OSA's Digital Library

Optics Express

Optics Express

  • Editor: Michael Duncan
  • Vol. 13, Iss. 13 — Jun. 27, 2005
  • pp: 4986–5012
« Show journal navigation

Quantum noise properties of parametric processes

C. J. McKinstrie, M. Yu, M. G. Raymer, and S. Radic  »View Author Affiliations


Optics Express, Vol. 13, Issue 13, pp. 4986-5012 (2005)
http://dx.doi.org/10.1364/OPEX.13.004986


View Full Text Article

Acrobat PDF (343 KB)





Browse Journals / Lookup Meetings

Browse by Journal and Year


   


Lookup Conference Papers

Close Browse Journals / Lookup Meetings

Article Tools

Share
Citations

Abstract

In this paper the quantum noise properties of phase-insensitive and phase-sensitive parametric processes are studied. Formulas for the field-quadrature and photon-number means and variances are derived, for processes that involve arbitrary numbers of modes. These quantities determine the signal-to-noise ratios associated with the direct and homodyne detection of optical signals. The consequences of the aforementioned formulas are described for frequency conversion, amplification, monitoring, and transmission through sequences of attenuators and amplifiers.

© 2005 Optical Society of America

1. Introduction

Four-wave-mixing (FWM) in a fiber, driven by one or two pump waves, makes possible the parametric amplification (PA) of an optical signal [1

1. K. O. Hill, D. C. Johnson, B. S. Kawasaki, and R. I. MacDonald, “CW three-wave mixing in single-mode optical fibers,” J. Appl. Phys. 49, 5098–5106 (1978). [CrossRef]

, 2

2. R. H. Stolen and J. E. Bjorkholm, “Parametric amplification and frequency conversion in optical fibers,” IEEE J. Quantum Electron. 18, 1062–1072 (1982). [CrossRef]

]. In this process, two pump photons are destroyed, and one signal and one idler photon are created: The signal wave is amplified and an idler wave is generated. Recent improvements in highly-nonlinear fibers have allowed parametric amplifiers (PAs) to produce high signal gains over broad signal-frequency bandwidths [3

3. J. Hansryd and P. A. Andrekson, “Broad-band continuous-wave pumped fiber optical parametric amplifier with 49-dB gain and wavelength-conversion efficiency,” IEEE Photon. Technol. Lett. 13, 194–191 (2001). [CrossRef]

, 4

4. S. Radic, C. J. McKinstrie, R. M. Jopson, Q. Lin, and G. P. Agrawal, “Record performance of a parametric amplifier constructed with highly-nonlinear fiber,” Electron. Lett. 39, 838–839 (2003). [CrossRef]

]. Another FWM process [5

5. K. Inoue, “Tunable and selective wavelength conversion using fiber four-wave mixing with two pump lights,” IEEE Photon. Technol. Lett. 6, 1451–1453 (1994). [CrossRef]

], in which one pump and one signal photon are destroyed, and one pump and one idler photon are created, makes possible tunable frequency conversion (FC), without gain, over broad bandwidths [6

6. K. Uesaka, K. K. Y. Wong, M. E. Marhic, and L. G. Kazovsky, “Wavelength exchange in a highly nonlinear dispersion-shifted fiber: theory and experiments,” IEEE J. Sel. Top. Quantum Electron. 8560–568 (2002). [CrossRef]

, 7

7. T. Tanemura, C. S. Goh, K. Kikuchi, and S. Y. Set, “Highly efficient arbitrary wavelength conversion within entire C-band based on nondegenerate fiber four-wave mixing,” IEEE Photon. Tech. Lett. 16, 551–553 (2004). [CrossRef]

]. Because of these demonstrated functionalities, parametric devices (PDs) are candidates for a variety of signal-processing applications [8

8. J. Hansryd, P. A. Andrekson, M. Westlund, J. Li, and P. O. Hedekvist, “Fiber-based optical parametric amplifiers and their applications,” IEEE J. Sel. Top. Quantum Electron. 8, 506–520 (2002). [CrossRef]

, 9

9. S. Radic and C. J. McKinstrie, “Two-pump fiber parametric amplifiers,” Opt. Fiber Technol. 9, 7–23 (2003). [CrossRef]

, 10

10. S. Radic and C. J. McKinstrie, “Optical parametric amplification and signal processing in highly-nonlinear fibers,” IEICE Trans. Electron. E88C, 859–869 (2005). [CrossRef]

].

PAs can be used to amplify optical signals before, during or after transmission through a fiber link. Because the idlers produced by PA, or FC, are frequency-shifted copies of the signals, by detecting the idlers one can monitor the signals without disrupting the flow of information. Transmission of the idlers, rather than the signals, makes possible frequency-dependent routing. Because the idlers produced by PA are phase-conjugate images of the signals, transmission of these idlers makes possible the reduction of impairments caused by phenomena such as pulse distortion, pulse arrival-time and phase jitter, and inter-pulse FWM. In the FWM processes that underly these applications, the powers of the output signals (idlers) do not depend on the phases of the input signals. Such processes are said to be phase insensitive (PI). One can make FWM processes phase sensitive (PS) by providing input idlers that beat with the signals, or choosing the pump and signal frequencies in ways that allow the signals to beat with themselves. The benefits of PS amplification include the reduction of noise, and pulse arrival-time and phase jitter, and the suppression of the modulation instability.

In the aforementioned applications, signal amplification and idler generation are accompanied by the addition of quantum-mechanical uncertainty (noise). Because these applications involve the transmission of information, it is important to determine the noise properties of the underlying parametric processes. In his classic review of the quantum-mechanical limits on noise production by linear amplifiers [11

11. C. M. Caves, “Quantum limits on noise in linear amplifiers,” Phys. Rev. D 26, 1817–1839 (1982). [CrossRef]

], Caves described the structure of many-mode amplification processes and derived formulas for the field-quadrature uncertainties associated with two-mode processes. (A mode is a frequency component of the electromagnetic field.) In this paper formulas are derived for the field-quadrature and photon-number uncertainties associated with many-mode parametric processes. The consequences of these formulas are described, for several applications of current interest.

2. Description and detection of light

The quantum-mechanical theory of light [12

12. W. H. Louisell, Radiation and Noise in Quantum Electronics (McGraw-Hill, 1964).

, 13

13. R. Loudon, The Quantum Theory of Light, 3rd Ed. (Oxford University Press, 2000).

] is formulated in terms of the photon-annihilation and -creation operators αj and αj , where j denotes a mode and † denotes a hermitian conjugate. These dimensionless mode operators obey the boson commutation relations [αj ;ak ]=0 and [αj ;ak ]=δjk .

The photon-number operator nj =aj αj . In DD a photodiode is used to measure the photon-number mean 〈nj ,〉 where 〈 〉 denotes an expectation value. The uncertainty in such a measurement is the photon-number variance 〈δnj2 〉=〈nj2 〉-〈nj2. For DD the SNR is 〈nj2/〈δnj2 〉.

The first quadrature operator qj (ϕ)=(αje -+aj e )/2, where ϕis a phase angle, and the second quadrature operator pj (ϕ)=qj (ϕ+π/2). If αj were a complex number, rather than an operator, qj and pj would be the real and imaginary parts of that number, measured in a coordinate system rotated by ϕ radians relative to the reference system. The quadrature operators obey the commutation relation [qj ; pj ]=i/2, which shows that they are conjugate operators (apart from factors of 21/2). The mean of the first quadrature is denoted by 
qj ‪ and the variance 
δqj2 ‪=
qj2 ‪-
qj ‪/2. Similar definitions apply to the second quadrature. It follows from the Heisenberg uncertainty principle that 
δqj2 ‪
δpj2 ‪≥1/16. States for which the equality sign applies are called minimal-uncertainty states: Coherent states have symmetric (circular) probability clouds, whereas squeezed states have asymmetric (elliptical) probability clouds.

aj(z)=μ̄(z)aj(0)+ν̄(z)ak(0),
(1)
ak(z)=ν̄*(z)aj(0)+μ̄*(z)ak(0).
(2)

The commutation relations [a 1;a1]=1 and [a 2;a2]=1 require the beam-splitter transfer functions µ̄ and ν̄ to satisfy the (same) auxiliary condition |µ̄|2+|ν̄|2=1. This condition ensures that the total photon-number is conserved. For reference, the functions |ν̄|2=T and |ν̄|2=1-T are called the transmittance and reflectance, respectively. By using DD at the output ports, one can measure the photon numbers nj and nk , and the photon-number difference djk =nj -nk . It follows from Eqs. (1) and (2) that

djk=(μ̄2ν̄2)(ajajakak)+2(μ̄ν̄*ajak+μ̄*ν̄ajak).
(3)

If the transmittance and reflectance are equal, the beam-splitter is said to be balanced.

In HD the mode to be measured (j) is combined with a local-oscillator (LO) mode (l) of the same frequency, before detection. It is customary to assume that the LO is a coherent state, for which al |αl 〈=αl /αl 〈, where the coherent-state parameter αl is a complex number. Let μ̄=μ̄eiϕμ̄,ν̄=νeiϕν̄, αl=αleiϕl and ak=aleiϕl. Then, for balanced HD, one can rewrite Eq. (3) in the simpler form

dj=ajaleiϕ+ajaleiϕ,
(4)

where the relative phase ϕ=ϕl -ϕµ ̄+ϕν ̄. Because the LO phase is included explicitly in Eq. (4), the LO eigenvalue equation is al |αl 〈=|αlαl 〈. It follows from Eq. (4) and the boson commutation relations that

dj(ϕ)=2αlqj(ϕ),
(5)
δdj2(ϕ)=4αl2δqj2(ϕ)+1lnj.
(6)

The subscript l in the last term in Eq. (6) indicates that it originates from the commutation relation [al ;al ]=1. For typical cases, in which the LO is much stronger than the measured mode (|αl |2≫〈nj 〉), the last term can be neglected. Thus, balanced HD measures the quadratures of mode j, with uncertainties that are characteristics of mode j, rather than the LO. For balanced HD the SNR is 〈dj2/〈δdj2 〉≈〈qj2/〈δqj2. Henceforth, for simplicity, ϕ will be called the LO phase. The measurement of optical fields is discussed in detail in [14

14. M. G. Raymer and M. Beck, “Experimental quantum state tomography of optical fields and ultrafast statistical sampling,” in Lecture Notes in Physics, Vol. 649, edited by M. Paris and J. Rehacek (Springer-Verlag, 2004), pp. 235–295.

].

3. Examples of parametric processes

In this section several examples of multiple-mode parametric interactions are described. PA driven by two pump waves (1 and 2) involves four product waves that are coupled by three distinct FWM processes, as illustrated in Fig. 1. Suppose that the signal frequency ω 1+=ω 1+ω, where ω is the modulation frequency, and let γ denote a photon. Then the modulation interaction (MI) in which 2γ 1γ 1_+γ 1+ produces an idler with frequency ω 1=ω 1-ω, the phase-conjugation (PC) process in which γ 1+γ 2 !γ 1++γ 2 produces an idler with frequency ω 2_=ω 2-ω and the Bragg scattering (BS), or FC, process in which γ 1++γ 2γ 1+γ 2+ produces an idler with frequency ω 2+=ω 2 +ω. It is customary to use a classical model for the strong (constant-amplitude) pumps and a quantal model for the weak (variable-amplitude) products (sidebands). In this approach, each of the preceding FWM processes involves two (interaction-picture) mode operators (one for each sideband). MI is characterized by the input-output relation

Fig. 1. Illustration of the constituent two-mode processes in a four-mode parametric interaction driven by two pump waves
a1+(z)=ν(z)a1(0)+μ(z)a1+(0).
(7)

The commutation relation [a 1+;a1+]=1 requires the MI transfer functions µ and ν to satisfy the auxiliary equation |µ|2-|ν|2=1. This condition ensures that transformation (7) is unitary.

A similar transformation characterizes the generation of the 1-idler. For reference, the functions |µ|2=G and |ν|2=G-1 are called the signal and idler gain, respectively. In quantum optics, transformation (7) is called a two-mode squeezing transformation [15

15. R. Loudon and P. L. Knight, “Squeezed light,” J. Mod. Opt. 34, 709–759 (1987). [CrossRef]

].

PC is characterized by the input-output relation

a1+(z)=μ(z)a1+(0)+ν(z)a2(0),
(8)

where the PC transfer functions µ and ν also satisfy the auxiliary equation |µ|2-|ν|2=1. A similar relation characterizes the generation of the 2- idler. Notice that Eq. (8) has the same form as Eq. (7).

BS is characterized by the input-output relation

a1+(z)=μ̄(z)a1+(0)+ν̄(z)a2+(0).
(9)

The BS transfer functions µ̄ and ν̄ satisfy the auxiliary condition |µ̄|2+|ν̄|2=1, which ensures that transformation (9) is unitary. A similar transformation characterizes the generation of the 2+ idler. For reference, the BS relations have the same form as the beam-splitter relations (1) and (2). Formulas for the MI, PC and BS transfer functions are stated in [16

16. C. J. McKinstrie, S. Radic, and M. G. Raymer, “Quantum noise properties of parametric amplifiers driven by two pump waves,” Opt. Express 12, 5037–5066 (2004). [CrossRef] [PubMed]

].

In a two-pump PA the aforementioned two-mode processes occur simultaneously. If one relabels the 1-, 1+, 2- and 2+ modes as 1, 2, 3 and 4, respectively, one can write the four-mode input-output relation in the form

a2(z)=v21(z)a1(0)+μ22(z)a2(0)+ν23(z)a3(0)+μ24(z)a4(0),
(10)

where the four-mode transfer functions satisfy the auxiliary equation -|µ 21|2+|µ 22|2-|ν 23|2+|µ 24|2=1. Similar relations characterize the idler-generation processes. Formulas for the four-mode transfer functions are stated in [16

16. C. J. McKinstrie, S. Radic, and M. G. Raymer, “Quantum noise properties of parametric amplifiers driven by two pump waves,” Opt. Express 12, 5037–5066 (2004). [CrossRef] [PubMed]

].

Fig. 2. Illustration of the architecture of one stage in a communication link with phase-insensitive amplification. The attenuator ◁ is followed by a parametric amplifier ▷. The signal, idler and scattered modes are labeled 1, 2r and 2r+1, respectively.

The loss process at the beginning of stage r is characterized by the input-output relation

a1(zr)=μ̄(zrzr1)a1(zr1)+ν̄(zrzr1)a2r+1(zr1),
(11)

where mode 1 is the signal, mode 2r+1 is the scattered mode associated with the loss mechanism, zr1 denotes the end of stage r-1 (beginning of stage r) and zr denotes the end of the fiber in stage r. The attenuator transfer functions µ̄ and ν̄ satisfy the auxiliary equation |µ̄|2+|ν̄|2=1. A similar relation characterizes the generation of the scattered mode, but is of lesser interest. For reference, the input-output relations for attenuators are identical to the relations for beam-splitters and frequency converters.

The gain process at the end of stage r is characterized by the input-output relation

a1(zr)=μ(zrzr)a1(zr)+ν(zrzr)a2r(zr),
(12)

where mode 2r is the idler, zr denotes the end of stage r and |µ|2-|ν|2=1. A similar relation characterizes the idler-generation process, but is of lesser interest. Equation (12) has the same form as Eqs. (7) and (8).

By combining Eqs. (11) and (12), one obtains the composite input-output relation

a1(zr)=μ11(zr,zr1)a1(zr1)+ν12r(zr,zr)a2r(zr)
+μ12r+1(zr,zr1)a2r+1(zr1),
(13)

a1(zs)=μ11(zs)a1(0)+r=1s[ν12r(zs)a2r(0)+μ12r+1(zs)a2r+1(0)].
(14)

For simplicity, in Eq. (14) the output point zs was denoted by zs and the input points of the idlers and scattered modes were denoted by 0. (One can formalize this relabeling of the input points by using step functions to extend the domains of the transfer functions.)

The idlers generated by PAs are frequency-shifted copies of the signals, and carry the same information. Consequently, by detecting only the generated idlers, one can access the information carried by the signals without disrupting the flow of information. In a real parametric monitor, coupling losses precede and follow the PA. Consequently, the input-output relation for the monitor [17

17. C. J. McKinstrie, S. Radic, R. M. Jopson, and A. R. Chraplyvy, “Quantum noise limits on optical monitoring with parametric devices,” submitted to Opt. Commun.

] has the same form as the relation for a two-stage link, in which the second PA is absent (G 2=1).

The aforementioned amplification processes (MI and PC) were PI, because the idler was generated within the amplifier, and the idler phase is determined by the phases of the pump(s) and signal. These processes become PS in the presence of an externally-generated idler (second signal) against which the (first) signal can beat [2

2. R. H. Stolen and J. E. Bjorkholm, “Parametric amplification and frequency conversion in optical fibers,” IEEE J. Quantum Electron. 18, 1062–1072 (1982). [CrossRef]

, 18

18. C. J. McKinstrie and S. Radic, “Phase-sensitive amplification in a fiber,” Opt. Express 12, 4973–4979 (2004). [CrossRef] [PubMed]

]. One can produce such an idler by using BS prior to MI or PC [18

18. C. J. McKinstrie and S. Radic, “Phase-sensitive amplification in a fiber,” Opt. Express 12, 4973–4979 (2004). [CrossRef] [PubMed]

, 19

19. C. J. McKinstrie, M. G. Raymer, S. Radic, and M. V. Vasilyev, “Quantum mechanics of phase-sensitive amplification in a fiber,” submitted to Opt. Commun.

].

As stated earlier, the PC process in which γ 1+γ 2γ 1+γ 2- involves waves whose frequencies satisfy the matching condition ω 1+ω 2=ω 1+ω 2. Equation (8) shows that the signal operator a 1+ is coupled to the idler operator a2. For the special case in which ω 1+ω 2=2ω 1+, which is illustrated in Fig. 3, the idler coincides with the signal and a 1+ is coupled to a1+ [18

18. C. J. McKinstrie and S. Radic, “Phase-sensitive amplification in a fiber,” Opt. Express 12, 4973–4979 (2004). [CrossRef] [PubMed]

, 19

19. C. J. McKinstrie, M. G. Raymer, S. Radic, and M. V. Vasilyev, “Quantum mechanics of phase-sensitive amplification in a fiber,” submitted to Opt. Commun.

]. If the pump frequencies are sufficiently far apart that dispersion prevents the 1- and 2+ idlers from interacting strongly with the 1+/2- signal, one can characterize this degenerate PC process by the input-output relation

a1+(z)=μ(z)a1+(0)+ν(z)a1+(0),
(15)

where the one-mode transfer functions µ and ν satisfy the auxiliary equation |µ|2-|ν|2=1. Formulas for these transfer functions are stated in [18

18. C. J. McKinstrie and S. Radic, “Phase-sensitive amplification in a fiber,” Opt. Express 12, 4973–4979 (2004). [CrossRef] [PubMed]

]. In quantum optics, transformation (15) is called a one-mode squeezing transformation [13

13. R. Loudon, The Quantum Theory of Light, 3rd Ed. (Oxford University Press, 2000).

, 15

15. R. Loudon and P. L. Knight, “Squeezed light,” J. Mod. Opt. 34, 709–759 (1987). [CrossRef]

]. It is intrinsically PS.

Fig. 3. Illustration of the constituent two-mode processes in a phase-sensitive parametric interaction driven by two pump waves.

Conversely, if the pump frequencies are not far apart, one must account for the idlers. As stated earlier, the MI of pump 1 couples a 1+ to a1. The BS process in which γ 1+γ 1+γ 1+γ 2 also couples a 1+ to a 1-. Likewise, the MI of pump 2, in which 2γ 2γ 1+ +γ 2+, couples a 1+ to a2+ and the BS process in which γ 1+ +γ 2γ 1+γ 2+ couples a 1+ to a 2+. If one relabels the 1-, 1+/2- and 2+ modes as 1, 2 and 3, respectively, one can write the three-mode input-output relation in the form

a2(z)=μ21(z)a1(0)+ν21(z)a1(0)+μ22(z)a2(0)
+ν22(z)a2(0)+μ23(z)a3(0)+ν23(0)a3(0),
(16)

where the three-mode transfer functions satisfy the auxiliary equation-|ν 21|2+|µ 21|2-|ν 22|2+|µ 22|2-|ν 23|2+|µ 23|2=1. The relations that characterize the idler-generation processes are similar, but not identical (a 1 is coupled to a3 by PC, but is not coupled to a 3, and a 3 is coupled to a1 by PC, but is not coupled to a 1).

Fig. 4. Illustration of the architecture of one stage in a communication link with phase-sensitive amplification. The attenuator ◁ is followed by a parametric amplifier▷. The signal and scattered modes are labeled 1 and r+1, respectively.
a1(zr)=μ̄(zrzr1)a1(zr1)+ν̄(zrzr1)ar+1(zr1),
(17)

which is equivalent to relation (11), and the gain process at the end of stage r is characterized by the input-output relation

a1(zr)=μ(zrzr)a1(zr)+ν(zrzr)a1(zr),
(18)

which is equivalent to relation (15). By combining Eqs. (17) and (18), one obtains the composite input-output relation

a1(zr)=μ11(zr,zr1)a1(zr1)+ν11(zr,zr1)a1(zr1)
+μ1r+1(zr,zr1)ar+1(zr1)+ν1r+1(zr,zr1)ar+1(zr1),
(19)

a1(zs)=μ11(zs)a1(0)+ν11(zs)a1(0)
+r=1s[μ1r+1(zs)ar+1(0)+ν1r+1(zs)ar+1(0)],
(20)

where the output point zs was denoted by zs and the input points of the scattered modes were denoted by 0.

4. Properties of parametric processes

aj(z)=k[μjk(z)ak(0)+νjk(z)ak(0)],
(21)

where the transfer functions µjk and νjk couple the output annihilation operator of mode j to the input annihilation and creation operators of mode k, respectively. The boson commutation relations, which are valid for all distances, imply that

l[μjl(z)νkl(z)μkl(z)νjl(z)]=0,
(22)
l[μjl(z)μkl*(z)νjl(z)νkl*(z)]=δjk.
(23)
l[μjl(z)2νjl(z)2]=1.
(24)

Suppose that the input signal is a coherent state with displacement (amplitude) αi (0). Then the input state |αi 〈=D(αi )|0〈, where D(αi ) is the displacement operator [13

13. R. Loudon, The Quantum Theory of Light, 3rd Ed. (Oxford University Press, 2000).

] and |0‹ is the vacuum state. It is customary to use the vacuum state as a virtual input state and incorporate the displacement required to produce the actual input state in the input-output relations associated with the process. By using the identity D (αi )αjD(αi )=αj +αiδij , one can rewrite the input-output relation (21) in the form

aj(z)=αj(z)+vj(z),
(25)

where the complex number

αj(z)=μji(z)αi(0)+vji(z)αi*(0)
(26)

is the output amplitude of mode j and the operator

vj(z)=k[μjk(z)ak(0)+vjk(z)ak(0)]
(27)

describes the effects of vacuum fluctuations on mode j. Because the vj operators only differ from the αj operators by complex numbers, the vj operators also must satisfy the boson commutation relations. The quadrature and number means and variances of mode j depend on the first-, second- and fourth-order moments of αj . The first-order moment is Eq. (25), from which it follows that

aj2=αj2+2αjvj+vj2,
(28)
ajaj=αj2+αjvj+αj*vj+vjvj,
(29)
ajaj=αj2+αjvj+αj*vj+vjvj,
(30)
(ajaj)2=αj4+[αj2(vj)2+αj2(vjvj+vjvj)+(αj*)2vj2]
+(vjvj)2+2αj2(αjvj+αj*vj)+2αj2vjvj
+(αjvj+αj*vj)vjvj+vjvj(αjvj+αj*vj).
(31)

Thus, to calculate the moments of αj , one must first calculate the moments of vj .

It follows from Eq. (27) that

vj0=kvjk1k,
(32)
vj0=kμjk*1k,
(33)

where |1 k 〈 represents a state with 1 photon in mode k and no photons in the other modes. Because different number states are orthogonal, Eqs. (32) and (33) imply that the first-order moments 〈vj 〉 and 〈vj 〉 are both zero. It follows from Eqs. (27), (32) and (33) that

vj20=k[μjkνjk0+212νjk22k+lkνjkνjl1k1l],
(34)
vjvj0=k[μjk20+212μjk*νjk2k+lkμjk*νjl1k1l],
(35)
vjvj0=k[212μjk*νjk2k+νjk20+lkμjl*νjk1k1l],
(36)
(vj)20=k[212(μjk*)22k+μjk*νjk*0+lkμjk*μjl*1k1l],
(37)

where |2 k 〉 represents a state with 2 photons in mode k and no photons in the other modes, and |1 k 1 l 〉 represents a state with 1 photon in mode k, one photon in mode l and no photons in the other modes. The second-order moments are all nonzero. Notice that 〈vj vj 〉-〈vj vj 〉=1, as it must. Because each state in Eqs. (34)(37) differs from the vacuum state by zero or two raising operations, each state in the third-order moment equations must differ from the vacuum state by one or three raising operations. Consequently, the third-order moments must all be zero. Because the operator vj vj is hermitian, one can deduce the fourth-order moment 〈(vj vj )2〉 from Eq. (36) and the identity ∑ klk µ* jl ν jk |1 k 1 l 〉=∑ kl>k(µ* jk νjl +µ* jl νjk )|1 k 1 l 〉.

By using the preceding results, one finds that the quadrature mean and variance are respectively. The quadrature mean depends on the output amplitude, which depends on the phases of the input signal and the transfer functions, and the LO phase. In contrast, the quadrature variance depends on the transfer functions and the LO phase, but not on the output amplitude. Let λjk =µjke -+ν* jke . Then Eq. (39) can be rewritten in the compact form

qj=(αjeiϕ+αj*eiϕ)2,
(38)
δqj2=[(kμjkνjk)ei2ϕ+k(μjk2+νjk2)+(kμjkνjk)*ei2ϕ]4,
(39)
δqj2=kλjk24.
(40)

The number mean and variance are

nj=αj2+kνjk2,
(41)
δnj2=αj2k(μjkνjk)*+αj2k(μjk2+νjk2)+(αj2)*kμjkνjk
+2kμjkνjk2+kl>kμjk*νjl+μjl*νjk2,
(42)

respectively. The number mean depends implicity on the phases of the input signal and the transfer functions. However, the number of noise photons ∑| k |νjk |2=∑ k |µjk |2-1 depends only on the magnitudes of the transfer coefficients. In contrast, the number variance depends on the phases of the output amplitude and the transfer coefficients. Let αj=αjeiϕj and λjk'=νjkeiϕj+ejk*eiϕj. (The definition of λjk differs slightly from the definition of λjk .) Then Eq. (42) can be rewritten in the compact form In the context of our model, which was described at the beginning of Section 3, Eqs. (38)(43) are exact.

δnj2=αj2kλjk'2+2kμjkνjk2+kl>kUjk*νjl+μjl*νjk2.
(43)

If there is more than one (coherent) input signal, the input state |{αi }〉=∏ iD(αi )|0〉. The output amplitude is defined by the equation

αj(z)=i[μji(z)αi(0)+νji(z)αi*(0)],
(44)

which is a generalization of Eq. (26). The vacuum operator is still defined by Eq. (27). Hence, the quadrature and number means and variances are given by Eqs. (38)(43), together with the modified amplitude equation (44). Other input states are considered briefly in Appendix A.

5. Selected applications

As stated in Section 2, the SNR associated with HD is 〈qj2/〈δqj2 〉, whereas the SNR associated with DD is 〈nj2/〈δnj2 〉. For a coherent input signal with state-parameter (amplitude) αi=αieiϕi, the quadrature mean 〈qi 〉=|αi |cos(ϕi -ϕ), where ϕi and ϕ are the input-signal and LO phases, respectively. The quadrature mean attains its maximal value |ai | when ϕ=ϕi , whereas the quadrature variance 〈δqi2 〉=1/4 for any value of ϕ. The photon-number mean 〈ni 〉=|αi |2 and variance 〈δni2 〉=|αi |2. Hence, for HD the maximal input-signal SNR

Si=4αi2,
(45)

whereas for DD the input-signal SNR

Si=αi2.
(46)

Although HD is more complicated than DD, it is more sensitive by a factor of 4 (6 dB).

The effects of parametric processes on the transmitted signal and generated idler(s) were determined in Section 4. It follows from Eqs. (38) and (40) that for HD the output SNR

Sj=4αj2cos2(ϕjϕ)kλjk2,
(47)

where αj=αjeiϕj is the output amplitude of mode j and λjk was defined before Eq. (40). As the following sections demonstrate, the SNR is often maximal when ϕ=ϕj . For these cases

Sj=4αj2kλjk2.
(48)

It follows from Eqs. (41) and (43) that for DD the SNRs

Sj=(αj2+kνjk2)2αj2kλjk'2+2kμjkνjk2+kl>kμjk*νjl+μjl*νjk2,
(49)

where λjk was defined before Eq. (43). For a many-photon input signal (|αi |2≫1), the stimulated terms in Eq. (48), which depend on the output strength |αj |2, are usually much larger that the spontaneous terms, which do not. For the usual cases

Sjαj2kλjk'2.
(50)

For each output mode (signal or idler) and detection method (HD or DD), the NF of the process is the SNR of the input signal divided by the SNR of the output mode.

5.1 Frequency conversion

The noise properties of PI convertors (or attenuators) and PI amplifiers were reviewed recently [16

16. C. J. McKinstrie, S. Radic, and M. G. Raymer, “Quantum noise properties of parametric amplifiers driven by two pump waves,” Opt. Express 12, 5037–5066 (2004). [CrossRef] [PubMed]

]. In Sections 5.1 and 5.2 these properties are described briefly, because they determine the properties of PI links, and contrast with the properties of PS devices and links.

Consider two-mode FC, which is made possible by BS (Fig. 1). Let the signal and idler modes be labeled 1 and 2, respectively, and suppose that the input signal is a coherent state with amplitude α1(0). Then it follows from the results of Section 4 that the output quantities αj (z)=µj 1 α 1(0), 〈qj (z)〉=|αj (z)|, 〈δqj2 (z)〉=1/4, 〈nj (z)〉=|αj (z)|2 and 〈δnj2 (z)〉=|αj (z)|2, where µ 11=µ̄, µ 21=-ν̄* and the LO phase ϕ=arg[αj (z)] is optimal. This standard FC process is PI, because the output photon-numbers (powers) of the signal and idler do not depend on the phase of the input signal.

The preceding results reflect the fact that the transmitted signal and generated idler are also coherent states. Hence, Eqs. (45) and (46) apply to HD and DD, respectively, with αi replaced by αj (z): HD is still more sensitive than DD by a factor of 4. The SNRs of the transmitted signal are reduced by the common factor 1=|µ̄|2, whereas the SNRs of the generated idler are lower than those of the input signal by the common factor 1=|ν̄|2. Because the SNRs associated with HD and DD are reduced by the same factors, the NFs associated with HD and DD are equal. The common NFs

F1(z)=1T,
(51)
F2(z)=1(1T),
(52)

where the transmittance T=|µ̄|2 is a periodic function of distance [16

16. C. J. McKinstrie, S. Radic, and M. G. Raymer, “Quantum noise properties of parametric amplifiers driven by two pump waves,” Opt. Express 12, 5037–5066 (2004). [CrossRef] [PubMed]

]. The signal and idler NFs are plotted as functions of the transmittance in Fig. 5. If T=1, F 1=1 (0 dB): The signal is transmitted perfectly and no idler is generated. Conversely, if T=0, F 2=1 (0 dB): No signal is transmitted and the generated idler is a perfect copy of the input signal.

If both modes have nonzero input amplitudes, the output modes are coherent states with amplitudes αj (z)=µ j1 α 1(0)+µ j2 α 2(0), where µ 12=ν̄ and µ 22=µ̄*. Let μ̄=μ̄eiϕμ̄ and ν̄=ν̄eiϕν̄. Then the output photon-numbers

α1(z)2=Tα12+(1T)α22+2[T(1T)]12α1α2cosξ,
(53)
α2(z)2=(1T)α12+Tα222[T(1T)]12α1α2cosξ,
(54)
Fig. 5. Noise figures [Eqs. (51) and (52)] plotted as functions of the transmittance T. The solid line represents the signal, whereas the dashed curve represents the idler.

where the relative phase ξ=ϕν ̄-ϕµ ̄+ϕ 2(0)-ϕ 1(0). On the right sides of Eqs. (53) and (54), αj is an abbreviation for αj (0). This alternative FC process is PS, because the output numbers of both modes depend on the phases of the input modes and transfer functions. However, Eqs. (45) and (46) still apply to HD and DD, respectively, with αi replaced by the PS αj (z), and the NFs associated with HD and DD are still equal. In Fig. 6 the signal and idler NFs are plotted as functions of the relative phase for the case in which |α 1|=|α 2| and T=0:5. Because of constructive interference, which allows one of the output amplitudes to be larger that the corresponding input amplitude, the NFs of the FC process can be less than 1 (0 dB). One could also define NFs based on the total input number, which would be greater than (or equal to) 1.

Fig. 6. Noise figures [Eqs. (45), (46), (53) and (54)] plotted as functions of the relative phase x. The solid line represents the signal, whereas the dashed curve represents the idler.

5.2 Phase-insensitive parametric amplification

Consider two-mode PA, which is made possible by MI or PC (Fig. 1). Let the signal and idler modes be labeled 1 and 2, respectively, and suppose that the input signal is a coherent state with amplitude α 1(0). Then it follows from the results of Section 4 that the output quantities α 1(z)=µ 11 α 1(0), µ 2(z)=ν 21 a 1* (0), 〈qj (z)〉=|αj (z)|, 〈δqj2 (z)〉=(|µjj |2+|νjk |2)/4,〈nj (z)〉=|αj (z)|2+|νjk |2 and 〈δnj2 (z)=|αj (z)|2(|µjj |2+|νjk |2)+|µjj νjk |2, where µ 11=µ=µ 22, ν 12=ν=ν 21, kj and the LO phase is optimal. This standard PA process is PI, because the output photon-numbers of the signal and idler do not depend on the phase of the input signal.

The preceding results show that the amplified signal and generated idler are not coherent states. For HD the SNRs

S1(z)=4Gn1(2G1),
(55)
S2(z)=4(G1)n1(2G1),
(56)

where the gain G=|µ|2 is a monotonically-increasing function of distance [16

16. C. J. McKinstrie, S. Radic, and M. G. Raymer, “Quantum noise properties of parametric amplifiers driven by two pump waves,” Opt. Express 12, 5037–5066 (2004). [CrossRef] [PubMed]

] and the input photon-number 〈n 1〉=|α 1(0)|2. By combining Eqs. (45), (55) and (56), one finds that the NFs

F1(z)=1+(G1)G,
(57)
F2(z)=1+G(G1).
(58)

For DD the SNRs

S1(z)=[Gn1+G1]2[G(2G1)n1+G(G1)],
(59)
S2(z)=[(G1)n1+G1]2[(G1)(2G1)n1+G(G1)].
(60)

Formulas (59) and (60) are valid for input signals with arbitrary numbers. However, current communication systems use many-photon input-signals, for which 〈n 1〉≫1. In this limit, the SNR formulas simplify and the NFs

F1(z)1+(G1)G,
(61)
F2(z)=1+G(G1).
(62)

Hence, for many-photon signals, the NFs associated with HD are the same as those associated with DD. The signal and idler NFs are plotted as functions of the gain in Fig. 7. In the high-gain limit (G≫1) the signal and idler NFs are both about 2 (3 dB). The degradation in signal quality is caused by the coupling of the signal to the (amplified) vacuum fluctuations associated with the idler.

Fig. 7. Noise figures [Eqs. (61) and (62)] plotted as functions of the gain G. The solid curve represents the signal, whereas the dashed curve represents the idler.

Now consider four-mode PA driven by two pumps (Fig. 1), and suppose that the input signal is a coherent state with amplitude ai (0). Then it follows from the results of Section 4 that the output quantities αj (z)=kji [(1-σ ji )αi (0)+σji αi * (0)], 〈qj (z)〉=|αj (z)|, 〈δqj2 (z)i=∑ k |kjk |2/4, 〈nj (z)〉=|αj (z)|2+∑ k |kjk |2σ jk and 〈δnj2 (z)〉=|αj (z)|2k |kjk |2+∑ kl>k|kjk kjl |2σ kl , where kjk =µjk if j and k are both odd, or even, kjk =νjk if one of j and k is odd and the other is even, σjk =0 if j and k are both odd, or even, σjk =1 if one of j and k is odd and the other is even, and the LO phase is optimal. The formulas for the photon-number mean and variance are consistent with Eqs. (122) and (123) of [16

16. C. J. McKinstrie, S. Radic, and M. G. Raymer, “Quantum noise properties of parametric amplifiers driven by two pump waves,” Opt. Express 12, 5037–5066 (2004). [CrossRef] [PubMed]

], which were derived by a different method.

For HD the SNRs and NFs

Sj(z)=4κji2nikκjk2,
(63)
Fj(z)=kκjk2κji2,
(64)

where 〈n 1〉=|αi (0)|2. For DD the SNRs

Sj(z)=[κji2ni+kκjk2σjk]2[κji2kκjk2ni+kl>kκjkκjl2σkl].
(65)

In the many-photon limit (〈ni 〉≫1), the SNR formulas simplify and the NFs

Fj(z)kκjk2κji2.
(66)

Hence, for many-photon signals, the NFs associated with HD are the same as those associated with DD.

The consequences of Eqs. (64) and (66) were described in detail in [16

16. C. J. McKinstrie, S. Radic, and M. G. Raymer, “Quantum noise properties of parametric amplifiers driven by two pump waves,” Opt. Express 12, 5037–5066 (2004). [CrossRef] [PubMed]

]. As a general rule, the signal and idler noise-levels increase in proportion to the number of modes that interact strongly. The interaction strengths (transfer functions |kjk |2) depend on the physical parameters associated with the pumps and signal, and the fiber. In some applications, such as optical switching [10

10. S. Radic and C. J. McKinstrie, “Optical parametric amplification and signal processing in highly-nonlinear fibers,” IEICE Trans. Electron. E88C, 859–869 (2005). [CrossRef]

], the pump frequencies are tuned in such a way that the output powers of the signals and idlers are comparable. The transfer functions |kjk |2 are also comparable , and (in fibers with random birefringence) the signal and idler NFs are closer to 6 dB than 0 dB (two-mode FC) or 3 dB (two-mode PA): Extra frequency diversity comes at the price of extra noise. However, if the pump frequencies are tuned in ways such that the PA or FC bandwidths are maximized, the signal is coupled strongly to the primary idler (which is generated by PC or BS, respectively), and is coupled weakly to the (other) secondary idlers. The signal and primary-idler NFs are only slightly higher than the NFs associated with the limiting two-mode processes: PA with signal and primary-idler NFs of about 3 dB, and FC with a primary-idler NF of about 0 dB, are possible [16

16. C. J. McKinstrie, S. Radic, and M. G. Raymer, “Quantum noise properties of parametric amplifiers driven by two pump waves,” Opt. Express 12, 5037–5066 (2004). [CrossRef] [PubMed]

]. PA with more than one input signal will be discussed in Section 5.5.

5.3 Transmission through a phase-insensitive link

For HD the SNR and NF

S1(z)=4GTn1(2G1),
(67)
F1(z)=(2G1)GT,
(68)

where the gain G=|µ|2, the attenuation (transmittance) T=|µ̄|2 and the input photon-number 〈n 1〉=|a 1(0)|2. Formula (67) has a simple physical interpretation: Attenuation transforms a coherent state with number 〈n 1〉 into a coherent state with number Tn 1〉, which is amplified subsequently. Hence, Eq. (67) is like Eq. (55), with a modified input number. For DD the SNR

S1(z)=[GTn1+G1]2[G(2G1)Tn1+G(G1)].
(69)

Equation (69) is like Eq. (59), with the input number 〈n 1〉 replaced by Thn 1i. For many-photon signals (Tn 1〉≫1), the NF

F1(z)(2G1)GT.
(70)

By combining the preceding results, one finds that for HD the SNR and NF

S1(z)=4n1[1+2s(G1)],
(71)
F1(z)=1+2s(G1).
(72)

Equations (71) and (72) are consistent with the results of [20

20. R. Loudon, “Theory of noise accumulation in linear optical-amplifier chains,” IEEE J. Quantum Electron. 21, 766–773 (1985). [CrossRef]

], which were obtained by a different method. In Eq. (72) one factor of s(G-1) comes from the |ν 12r|2 terms, whereas the other comes from the |α 12r+1|2 terms. Because the latter terms are only nonzero if ν̄ is nonzero (|µ̄|<1), one can conclude that attenuation and amplification both degrade the signal quality. For DD the SNR

S1(z)=[n1+s(G1)]2{[1+2s(G1)]n1+s(G1)[1+s(G1)]}.
(73)

Equation (73) is consistent with Eqs. (47) and (48) of [17

17. C. J. McKinstrie, S. Radic, R. M. Jopson, and A. R. Chraplyvy, “Quantum noise limits on optical monitoring with parametric devices,” submitted to Opt. Commun.

], and the results of [20

20. R. Loudon, “Theory of noise accumulation in linear optical-amplifier chains,” IEEE J. Quantum Electron. 21, 766–773 (1985). [CrossRef]

], which were obtained by different methods. For many-photon signals [〈n 1〉≫s(G-1)], the NF

F1=1+2s(G1).
(74)

Hence, for many-photon signals, the NF associated with HD is the same as that associated with DD. In the high-gain limit the NF is about 2sG.

5.4 Phase-insensitive parametric monitoring.

Consider the transmission of a signal by a PI monitor. As stated in Section 3, the input-output relation for a monitor, with coupling losses before and after the PA, has the same form as the relation for a two-stage link, in which the second PA is absent (Fig. 2). Let the signal and idler modes be labeled 1 and 2, respectively, and let the scattered modes be labeled 3 and 5. Then it follows from the results of Section 4 (and Appendix B) that α 1(z)=k 1 α 1(0), 〈q 1(z)〉=|α 1(z)|, 〈δq12(z)〉=(|k 1|2+|k 2|2+|k 3|2+|k 5|2)=4, 〈n 1(z)〉=|α 1(z)|2+|k 2|2 and 〈δn12(z)〉=|α 1(z)|2(|k 1|2+|k 2|2+|k 3|2+|k 5|2)+|k 1 k 2|2+|k 2 k 3|2+|k 2 k 5|2, where k 1=µ̄ fµµ̄i , k 2=µ̄ f ν, k 3=µ̄ fµ ν̄ f 〉, k 5=ν̄ f and the LO phase is optimal. The subscripts i and f denote the initial loss (in stage 1) and the final loss (in stage 2), respectively.

For HD the SNR and NF

S1(z)=4TfGTin1[1+2Tf(G1)],
(75)
F1(z)=[1+2Tf(G1)](TfGTi),
(76)

where the gain G=|µ|2, the transmittances Ti =|µ̄ i |2 and Tf =|µ̄ f |2, and the input photon-number 〈n 1〉=|α 1(0)|2. For DD the SNR

S1(z)=[TfGTin1+Tf(G1)]2{(TfGTi)[1+2Tf(G1)]n1
+Tf(G1)[1+Tf(G1)]}.
(77)

In the many-photon limit (Tin 1〉≫1), the SNR formula simplifies and the NF

F1(z)[1+2Tf(G1)](TfGTi).
(78)

The results of Sections 5.1–5.4 show that the NFs associated with HD and DD are always equal for PI processes with one many-photon input signal.

5.5 Phase-sensitive parametric amplification

The noise properties of PS frequency down-convertors were reviewed in [13

13. R. Loudon, The Quantum Theory of Light, 3rd Ed. (Oxford University Press, 2000).

, 15

15. R. Loudon and P. L. Knight, “Squeezed light,” J. Mod. Opt. 34, 709–759 (1987). [CrossRef]

] and the noise properties of PS amplifiers were reviewed in [18

18. C. J. McKinstrie and S. Radic, “Phase-sensitive amplification in a fiber,” Opt. Express 12, 4973–4979 (2004). [CrossRef] [PubMed]

, 19

19. C. J. McKinstrie, M. G. Raymer, S. Radic, and M. V. Vasilyev, “Quantum mechanics of phase-sensitive amplification in a fiber,” submitted to Opt. Commun.

]. In Section 5.5 the latter properties are described briefly, because they determine the properties of PS links, and contrast with the properties of PI devices and links.

Consider the degenerate PC process in which a signal is amplified by two pumps, whose frequencies differ from the signal frequency by equal and opposite amounts (Fig. 3). This frequency condition allows the signal to interact with itself, rather than an idler. Let the signal mode be labeled 1. Then it follows from the results of Section 4 that α 1(z)=µα 1(0)+να*1(0), 〉q 1(z)〉=|α 1(z)|cos[ϕ 1(z)-ϕ], 〈δq12(z)〉=|λ|2/4, 〈ν 1(z)〉=|α 1(z)|2+|ν|2 and 〈δn12(z)〉=|α 1(z)|2|λ |2+2|µν|2, where ϕ 1(z)=arg[α 1(z)] is the output phase, ϕ is the LO phase, λ=µe -+ν*e and λ'=μeiϕ1+ν*eiϕ1. Let μ=μeiϕμ and ν=νeiϕν. Then the output strength and phase

α1(z)2=α1(0)2{2G1+2[G(G1)]12cosξ},
(79)
ϕ1(z)=ϕ1(0)+ϕμ+tan1[(G1)12sinξG12+(G1)12cosξ],
(80)

where the PI gain G=|µ|2 is a monotonically-increasing function of distance [18

18. C. J. McKinstrie and S. Radic, “Phase-sensitive amplification in a fiber,” Opt. Express 12, 4973–4979 (2004). [CrossRef] [PubMed]

] and the relative phase ξ=ϕν -ϕµ -2ϕ 1(0). It is convenient to define the PS gain-function H(ξ)=2G-1+2[G(G-1)]1/2 cosξ. The output photon-number

n1(z)=H(ξ)n1+G1,
(81)

where 〈n 1〈=|α 1(0)|2, and the output quadrature- and number-variances

δq12(z)=H(η)4,
(82)
δn12(z)=H(ξ)H(ζ)n1+2G(G1),
(83)

where the relative phases η=ϕv +ϕµ -2ϕ and ζ=ϕv +ϕµ -2ϕ 1(z). Notice that ξ-η=2[ϕ-ϕ 1(z)]. It follows from Eq. (80) and the definition of ζ that

ζ=ξtan1[(G1)12sinξG12+(G1)12cosξ].
(84)

The output strength, phase, number and number-variance are all controlled by the relative phase ϕν -ϕµ -2ϕ 1(0), which depends on the coupling phases ϕµ and νv , and the input phase ϕ 1(0).

In contrast, the output quadrature-variance is controlled by the relative phase ϕν +ϕµ -2ϕ, which depends on the coupling phases and the LO phase ϕ, but not the input phase. These phase dependences were illustrated in [19

19. C. J. McKinstrie, M. G. Raymer, S. Radic, and M. V. Vasilyev, “Quantum mechanics of phase-sensitive amplification in a fiber,” submitted to Opt. Commun.

].

S1(z)=4n1H(ξ)cos2[(ζη)2]H(η),
(85)
F1(z)=H(η){H(ξ)cos2[(ζη)2]},
(86)

whereas for DD the SNR

S1(z)=[H(ξ)n1+G1]2[H(ξ)H(ζ)n1+2G(G1)].
(87)

In the many-photon limit (〈n 1≫1), the SNR formula simplifies and the NF

F1(z)H(ζ)H(ξ).
(88)

As noted after Eq. (83), one can obtain z from η by replacing the LO phase with the output phase, in which case formula (86) reduces to formula (88): One can consider DD as self-homodyning detection.

In Fig. 8 the NF associated with HD is plotted as a function of ξ and η, for the case in which G=10. The region of Fig. 8a in which the contours merge (ηπ) is magnified in Fig. 8b.

Fig. 8. Homodyne noise-figure [Eq. (86)] plotted as a function of the input phase ξ and the local-oscillator phase η. Dark shadings denote low noise figures, whereas light shadings denote high noise figures. The contour spacing is 4 dB.

With the exception of this narrow region, the NF contours are almost vertical: The NF is almost independent of η. This behavior has a simple explanation: When a signal is subject to PS amplification, its in-phase component is amplified, whereas its out-of-phase component is attenuated. Hence, in the high-gain regime, the output signal is predominantly in-phase (ζ≈0 or 2π). For the same reason, the in-phase axis of the probability cloud that characterizes the (initially-coherent) signal fluctuations is stretched, whereas the out-of-phase axis is squeezed. As one varies the LO phase (quadrature-measurement axis), the measured signal-strength decreases at almost the same rate as the (squared) width of the probability cloud. Hence, the NF is almost independent of η. For most values of η, the NF is maximal when ξ≈π, because the signal strength is minimal. In Fig. 9 the NF associated with HD is plotted as a function ξ, and as a function of η, for cases in which G=10.

Fig. 9. Homodyne noise-figure [Eq. (86)] plotted as a function of (a) the input phase ξ, for the case in which the local-oscillator phase η=0, and (b) η, for the case in which ξ=0.

In Fig. 10 the NF associated with DD is plotted as a function of ξ, for the case in which G=10 and 〈n 1〉=100. The approximate formula (88) predicts the NF accurately, provided that the signal is amplified significantly (ξ≠π).

Fig. 10. Direct noise-figure plotted as a function of the input phase ξ. The solid curve represents the exact noise figure [Eqs. (46) and (87)], whereas the dashed curve represents the approximate noise figure [Eq. (88)].

Now consider two-mode PA, which is made possible by MI or PC (Fig. 1). If both modes have nonzero input amplitudes, the output amplitudes αj (z)=µjjαj (0)+νjkα* k (0), where µjj =µ, νjk =ν and kj. It follows from the results of Section 4 that 〈qj (z)〈=|αj (z)|cos[ϕj (z)-ϕ], 〈ξqj2 (z)〉=(2G-1)/4, 〈nj (z)〉=|αj (z)|2+G-1 and 〈δnj2 (z)〉=|αj (z)2(2G-1)+G(G-1), where the PI gain G=|µ|2. This alternative PA process is PS [2

2. R. H. Stolen and J. E. Bjorkholm, “Parametric amplification and frequency conversion in optical fibers,” IEEE J. Quantum Electron. 18, 1062–1072 (1982). [CrossRef]

], because the output photon-numbers of both modes depend on the phases of the input modes and transfer functions. The quadrature mean attains its maximal value |αj (z)| when ϕ=ϕj (z), whereas the quadrature variance does not depend on ϕ. The output strengths

α1(z)2=Gα12+(G1)α22+2[G(G1)]12α1α2cosξ,
(89)
α2(z)2=(G1)α12+Gα22+2[G(G1)]12α1α2cosξ,
(90)

where the relative phase ξ=ϕν -ϕµ -ϕ 2(0)-ϕ 1(0). On the right sides of Eqs. (89) and (90), αj is an abbreviation for αj (0).

For HD the SNRs and NFs

Sj(z)=4αj(z)2(2G1),
(91)
Fj(2)=(2G1)αj(0)αj(z)2,
(92)

whereas for DD the SNRs

Sj(z)=[[αj(z)]2+G1]2[(2G1)αj(z)2+G(G1)].
(93)

In the many-photon limit (|αj (z)|2G-1), the SNR formulas simplify and the NFs

Fj(z)(2G1)αj(0)αj(z)2.
(94)

Hence, for many-photon inputs, the NFs associated with HD are the same as those associated with DD.

In Fig. 11 the NF associated with DD is plotted as a function of the relative phase for the case in which G=10 and |α 1(0)|2=100=|α 2(0)|2 (and the signal and idler NFs are equal). Because of constructive interference, the common NF of this alternative PA process can be less than 1 (0 dB). The approximate formula (94) predicts the NF accurately, provided that the input modes are amplified significantly (ξ≠π). The dashed curve in Fig. 11 also represents the common NF associated with HD. The noise properties of four-mode PA with two nonzero input amplitudes are similar.

Fig. 11. Direct noise-figure plotted as a function of the relative phase x. The solid curve represents the exact noise figure [Eqs. (46) and (93)], whereas the dashed curve represents the approximate noise figure [Eq. (94)].

The degenerate PC process produces an output signal whose strength depends on the input phase ϕ 1(0), and whose quadrature mean and variance both depend on the LO phase ϕ. These properties typify a one-mode squeezing transformation [13

13. R. Loudon, The Quantum Theory of Light, 3rd Ed. (Oxford University Press, 2000).

, 15

15. R. Loudon and P. L. Knight, “Squeezed light,” J. Mod. Opt. 34, 709–759 (1987). [CrossRef]

]. The PA process with two input modes also produces output modes whose strengths depend on the input phases ϕ 1(0) and ϕ 2(0), and whose quadrature means depend on ϕ. However, the quadrature variances of the output modes are independent of ϕ: Neither mode is squeezed by itself. Although the output modes are not squeezed, they are correlated: By using the FC process to combine them, one can produce new output modes that are squeezed [18

18. C. J. McKinstrie and S. Radic, “Phase-sensitive amplification in a fiber,” Opt. Express 12, 4973–4979 (2004). [CrossRef] [PubMed]

, 19

19. C. J. McKinstrie, M. G. Raymer, S. Radic, and M. V. Vasilyev, “Quantum mechanics of phase-sensitive amplification in a fiber,” submitted to Opt. Commun.

]. These properties typify a two-mode squeezing transformation [15

15. R. Loudon and P. L. Knight, “Squeezed light,” J. Mod. Opt. 34, 709–759 (1987). [CrossRef]

].

5.6 Transmission through a phase-sensitive link

α1(z)2=Tα1(0)2{2G1+2[G(G1)]12cosξ},
(95)
ϕ1(z)=ϕ1(0)+ϕμ+ϕμ̄+tan1[(G1)12sinξG12+(G1)12cosξ],
(96)

where the PI gain G=|µ|2, the attenuation (transmittance) T=|µ̄|2 and the relative phase ξ=ϕν -ϕµ -2[ϕ 1(0)+ϕµ ̄]. It is convenient to define the PS gain-function H(ξ)=2G-1+2[G(G-1)]1/2 cosξ. The output photon-number

n1(z)=H(ξ)Tn1+G1,
(97)

where the input number 〈n 1〉=|α 1(0)|2, and the output quadrature- and number-variances

δq12(z)=H(η)4,
(98)
δn12(z)=H(ξ)H(ζ)Tn1+2G(G1),
(99)

For HD the SNR and NF

S1(z)=4Tn1H(ξ)cos2[(ζη)2]H(η),
(100)
F1(z)=H(η){H(ξ)Tcos2[(ζη)2]},
(101)

whereas for DD the SNR

S1(z)=[H(ξ)Tn1+G1]2[H(ξ)H(ζ)Tn1+2G(G1)].
(102)

In the many-photon limit (〈n 1≫1), the SNR formula simplifies and the NF

F1(z)H(ζ)[H(ξ)T].
(103)

By combining Eqs. (26), (38) and (40) with the preceding formulas for |µ 1k+ν 1k|2, one finds that for HD the SNR and NF

S1(z)=4α1(0)2[1+s(L1)],
(104)
F1(z)=1+s(L1).
(105)

Equations (104) and (105) are consistent with the results of [20

20. R. Loudon, “Theory of noise accumulation in linear optical-amplifier chains,” IEEE J. Quantum Electron. 21, 766–773 (1985). [CrossRef]

], which were obtained by a different method. By combining Eqs. (41) and (43) with the formulas for µ 1k and ν 1k (as detailed in Appendix C), one finds that for DD the SNR

S1(z){α1(0)2+[s(L1)1]4}2[1+s(L1)]α1(0)2+{[1+s(L1)]22}8.
(106)

F1(z)1+s(L1).
(107)

6. Summary

In fiber optics, a process is termed phase-sensitive (PS) if the power of the output signal depends on the phase of the input signal. Otherwise, it is termed phase-insensitive (PI). In quantum optics, the term PS (PI) is used to describe a process in which the quadrature variance of the output signal depends (does not depend) on the phase of the local oscillator (LO) used to measure it. To avoid confusion, we term such a process isotropic (anisotropic).

All of the PI processes considered herein are isotropic (one-input-mode FC and PA, PI monitoring and transmission through a PI link), as are the processes that are made PS by the presence of a second input mode (two-input-mode FC and PA). For an isotropic process, the SNR associated with HD is maximal when the LO phase equals the relevant output phase (signal or idler), in which case the SNR is given by Eq. (48), with λ jk =µjk or ν* jk . For a many-photon signal, the spontaneous contributions to the photon-number mean and variance are negligible, in which case the SNR associated with DD is given by Eq. (50), with λjk =µjk or ν* jk . Hence, for isotropic processes with coherent many-photon input signals, the input and output SNRs associated with HD are larger than those associated with DD by a factor of 4 (6 dB). The noise figure (NF) of a parametric process is the SNR of the input signal divided by the SNR of the relevant output mode (signal or idler). For isotropic processes with many-photon signals, the NFs associated with HD and DD are equal. Two of the PS processes considered herein (PS amplification and transmission through a PS link) are anisotropic. In the high-gain limit, the signal SNR associated with HD is maximal when the LO phase equals the signal phase, in which case it is given by Eq. (48), with λjk =λjk . The SNR depends only weakly on the LO phase. For a many-photon signal, the spontaneous contributions to the photon-number mean and variance are negligible, in which case the SNR associated with DD is given by Eq. (50). Hence, for anisotropic processes with coherent many-photon input signals and high gains, the input and output SNRs associated with HD are larger than those associated with DD by a factor of 4 (6 dB), so the NFs associated with HD and DD are equal. These results allow the term NF to be used unambiguously. The preceding statements were based on one-time measurements of signals. Many-time measurements of signals [14

14. M. G. Raymer and M. Beck, “Experimental quantum state tomography of optical fields and ultrafast statistical sampling,” in Lecture Notes in Physics, Vol. 649, edited by M. Paris and J. Rehacek (Springer-Verlag, 2004), pp. 235–295.

], and joint measurements of signals and correlated idlers [15

15. R. Loudon and P. L. Knight, “Squeezed light,” J. Mod. Opt. 34, 709–759 (1987). [CrossRef]

], were not considered.

For one-input-mode FC (Section 5.1), the signal NF varies from 1 (0 dB) to ∞, whereas the idler NF varies from ∞ to 1: It is possible to generate an idler that is a perfect copy of the input signal. For two-mode FC (Section 5.1), constructive interference allows the standard NFs to be less than 1. If the input numbers are equal, the minimal NFs are 1/2 (-3 dB). However, if one were to define alternative NFs based on the total input number, the minimal NFs would be 1. These results reflect the fact that the FC images of coherent states are also coherent states.

For one-input-mode PA (Section 5.2), the signal NF varies from 1 (0 dB) to 2 (3 dB), whereas the idler NF varies from ∞ to 2. In the high-gain limit, both NFs are about 2. The degradation in signal quality is caused by the coupling of the signal to the (amplified) vacuum fluctuations associated with the idler. For two-input-mode PA (Section 5.5), constructive interference allows the standard signal and idler NFs to be less than 1. If the input numbers are equal, the minimal NFs are 1/2 (-3 dB). However, if one were to define alternative NFs based on the total input number, the minimal NFs would be 1 (0 dB). Many-mode PI processes (Section 5.2) were discussed in [16

16. C. J. McKinstrie, S. Radic, and M. G. Raymer, “Quantum noise properties of parametric amplifiers driven by two pump waves,” Opt. Express 12, 5037–5066 (2004). [CrossRef] [PubMed]

]. In general, the presence of extra idlers increases the signal and idler NFs (relative to those of two-mode FC and PA).

PS amplification in a fiber occurs when the signal frequency is the average of the two pump frequencies. This frequency condition allows the signal to interact with itself, rather than an idler: No vacuum fluctuations are coupled to the signal. For in-phase amplification (Section 5.5), the signal NF is 1 (0 dB), because the mean input-signal and the in-phase component of the (coherent) input-signal fluctuations are amplified by the same amount. An out-of-phase signal is attenuated.

In this paper a formalism was developed to determine the noise properties of parametric processes; those of current interest (described above) and those yet to be imagined. The results of this paper apply to interactions between discrete modes. Interactions between modes with continuous frequency spectra will be described elsewhere.

Appendix A: Arbitrary input states

In Section 4 formulas for the quadrature and number means and variances were derived for coherent input states. In this appendix formulas are derived for arbitrary input states. First, suppose that there is only a single input mode, which, without loss of generality, is labeled 1. Then one can rewrite the input-output relation (21) in the form

aj(z)=uj(z)+vj(z),
(108)

where the output operator

uj(z)=μj1(z)a1(0)+νj1(z)a1(0)
(109)

describes the effects of the input mode and the output operator

vj(z)=k>1[μjk(z)ak(0)+νjk(z)ak(0)]
(110)

describes the effects of vacuum fluctuations.

To determine the quadrature and number means and variances, one must first calculate the lower-order moments of the output operator. The first-order moment is Eq. (108), the second-order moments are

aj2=uj2+2ujvj+vj2,
(111)
ajaj=ujuj+ujvj+ujvj+vjvj,
(112)
ajaj=ujuj+ujvj+ujvj+vjvj,
(113)

and the fourth-order moment is

(ajaj)2=(ujuj)2+[uj2(vj)2+ujujvjvj+ujujvjvj+(uj)2vj2]
+(vjvj)2+ujuj(ujvj+ujvj)+(ujvj+ujvj)ujuj
+2ujujvjvj+(ujvj+ujvj)vjvj+vjvj(ujvj+ujvj).
(114)

The moments of vj were evaluated in Section 4. Because the (expectation values of the) first-and third-order moments of vj are zero, the first-order moment of αj is determined solely by uj , the contributions of uj and vj to the second-order moments add independently, and the fourth, fifth, seventh and eighth terms on the right side of Eq. (114) are zero. It follows from Eq. (108), Eqs. (111)(113) and these observations, that the quadrature mean and variance

qj=ujeiϕ+ujeiϕ2,
(115)
δqj2=δq2(uj)+δq2(vj),
(116)

where 〈δq 2(uj )〉=〈q 2(uj )〉-〈q(uj )〉2 is the variance contribution from uj and

δq2(vj)=k>1λjk24,
(117)

where λjk =µjke -+ν* jke , is the other variance contribution. It follows from Eqs. (113) and (114), and the preceding observations, that the number mean and variance

nj=ujuj+vjvj,
(118)
δnj2=δn2(uj)+uj2(vj)2+ujujvjvj
+ujujvjvj+(uj)2vj2+δn2(vj),
(119)

where 〈δn 2(uj )〉=〈n 2(uj )〉-〈n(uj )〉2 is the variance contribution from uj , the second-order moments

vj2=k>1μjkνjk,
(120)
vjvj=k>1μjk2,
(121)
vjvj=k>1νjk2,
(122)
(vj)2=k>1μjk*νjk*
(123)

and the other variance contribution

δn2(vj)=2k>1μjkνjk2+k>1l>kμjk*νjl+μjl*νjk2.
(124)

Further progress requires the specification of the input state. In the absence of such a specification, all one can do is demonstrate that the preceding results are consistent with the results of Section 4. If the input state 1 is a coherent state, Eqs. (38)(43) apply to the moments of uj , with k=1. It follows from this observation that

q(uj)=(αjeiϕ+αj*eiϕ)2,
(125)
δq2(uj)=λj124,
(126)

where αj =µj 1 α 1+ν j1 α*1 and λ j1=µ j1 e -+ν*j1 e . Equation (125) is identical to Eq. (38). By combining Eqs. (116), (117) and (126), one obtains Eq. (40). It also follows from the preceding observation that

n(uj)=αj2+νj12,
(127)
δn2(uj)=αj2λj1'2+2μj1νj12,
(128)

where λj1'=μj1eiϕj+νj1*eiϕj and ϕj =arg(αj ). By combining Eqs. (118), (122) and (127), one obtains Eq. (41). It follows from Eqs. (119)(124) and Eq. (128) that

δnj2=αj2λj1'2+2μj1νj12
+(αj2+μj1νj1)k>1(μjkνjk)*+(αj2+μj12)k>1νjk2
+(αj2+νj12)k>1μjk2+(αj2+μj1νj1)*k>1μjkνjk
+2k>1μjkνjk2+k>1l>kμjk*νjl+μjl*νjk2.
(129)
αj2λjk'2=αj2μjk*νjk*+αj2μjk2+αj2νjk2+(αj*)2μjkνjk,
(130)
μj1*νjl+μjl*νj12=μj1νj1μjl*νjl*+μj12νjl2+μjl2νj12+μj1*νj1*μjlνjl,
(131)

one can show that Eq. (129) is equivalent to Eq. (43).

Second, suppose that there are multiple input modes, which are labeled by the subscript i. Then one can rewrite the input-output relation in the form of Eq. (108), in which the output operators

uj(z)=j[μjl(z)ai(0)+νji(z)ai(0)],
(132)
vj(z)=ki[μjk(z)ak(0)+μjk(z)ak(0)].
(133)

The quadrature and number means and variances are still given by Eqs. (115), (116), (118) and (119), in which the moments and variance contribution of vj are given by truncated versions of Eqs. (120)(124). Once again, further progress requires the specification of the input states.

Appendix B: Phase-insensitive link

a1(z1")=μμ̄a1(z0)+νa2(z'1)+μν̄a3(z0).
(134)

It follows from Eqs. (13) and (134) that, for a two-stage link,

a1(z2)=(μμ̄)2a1(z0)+(μμ̄)νa2(z1)+(μμ̄)μν̄a3(z0)+νa4(z2)+μν̄a5(z1).
(135)

By iterating Eq. (13) s times, one finds that

a1(zs")=(μμ̄)sa1(z0)+r=1s(μμ̄)sr[νa2r(z'r)+μν̄a2r+1(z"r1)].
(136)

Thus, µ 11=(µµ̄) s , ν 12r=(µµ̄) s-r ν and µ 12r+1=(µµ̄)s-r µν̄, as stated in Section 5.3.

To derive the SNRs (71) and (73), one must evaluate the sums ∑ k |kk |2 and ∑ kl>k|kkkl |2σ kl , where σ kl =0 if k and l are both odd, or even, and σ kl =1 if one of k and l is odd and the other is even. For a balanced link, |k 1|2=1 and |kk |2=G-1 if k>1. It follows from these facts that the first sum ∑ k |kk |2=1+2s(G-1), as stated in Eqs. (71) and (73). The second sum ∑ kl>k|kkkl |2σ kl is evaluated as follows: For stage 0 (k=1) there are s contributions of the form |k 1 kl |2=1(G-1), which sum to s(G-1). For stage 1 (k=2 and 3) there are s contributions of the form |k 2 kl |2=(G-1)2 and s-1 contributions of the form |k 3 kl |2=(G-1)2, which sum to (2s-1)(G-1)2. For stage 2 (k=4 and 5) there are s-1 contributions of the form |k 4 kl |2=(G-1)2 and s-2 contributions of the form |k 5 kl |2=(G-1)2, which sum to (2s-3)(G-1)2. By continuing this counting process, one finds that the second sum is s(G-1)+r=1s[2(s-r)+1](G-1)2=s(G-1)[1+s(G-1)], as stated in Eq. (73).

Appendix C: Phase-sensitive link

Consider the transmission of a signal through a PS link. For a one-stage link, Eq. (19) states that

a1(z1")=μ̄μa1(z0")+μ̄*νa1(z0")+ν̄μa2(z0")+ν̄*νa2(z0").
(137)

For the case considered in the text, µ, ν, µ̄ and ν̄ are real. It follows from Eqs. (19) and (137) that, for a two-stage link,

a1(z2)=μ̄2(μ2+ν2)a1(z0)+μ̄2(2μν)a1(z0)+μ̄ν̄(μ2+ν2)a2(z0)
+μ̄ν̄(2μν)a2(z0)+ν̄μa3(z1")+ν̄νa3(z1").
(138)

By iterating Eq. (19) s times, one finds that

a1(z2")=μ̄s[ps(μ,ν)a1(z0")+qs(μ,ν)a1(z0")]+r=1sμ̄srν̄
×[ps+1r(μ,ν)ar+1(zr1)+qs+1r(μ,ν)ar+1(zr1)],
(139)

To derive the SNRs (104) and (106), one must evaluate the sums ∑ k |λ 1k|2 and ∑ k |λ1k|2, where λ 1k=µ 1k e -+ν*1k e and λ'1k=μ1keiϕ1+ν1k*eiϕ1. For the in-phase quadrature, ϕ=0. It follows from the results of the preceding paragraph that |λ 11|2=1 and |λ 1r+1|2=L-1. Thus, r=0s|λ 1r+1(0)|2=1+s(L-1), as stated in Eq. (104): The in-phase sum (quadrature variance) increases monotonically as the number of stages increases. For the case considered, in which ϕ 1(z)=0, λ1r+1=λ 1r+1, so r=0s|λ1r+1|2=1+s(L-1), as stated in Eq. (106). For the out-of-phase quadrature ϕ=π/2. It follows from the results of the preceding paragraph that |λ 11|2=T 2s and |λ 1r+1|2=T(1-T)T 2s-2r. Thus, r=0s|λ 1r+1(π/2)|2=(T+T 2s)/(1+T): As the number of stages increases, the out-of-phase sum (quadrature variance) tends quickly to its limit T/(1+T). It follows from Eq. (40), the definition of λ 1k, and the assumption that µ 1k and ν 1k are real, that 〈δq12(ϕ)〉=〈δq12(0)〉cos2 ϕ+〈δq12(π/2)sin2 ϕ. Because the in-phase variance is much larger then the out-of-phase variance, 〈δq12(ϕ)〉≈〈δq12(0)〉cos2 ϕ. Recall that 〈q 1(ϕ)〉2=|α 1(0)|2 cos2 ϕ. By combining these results, one finds that the SNR associated with HD depends weakly on ϕ, and in-phase measurement (ϕ=0) is optimal.

To derive the SNR (106), one must evaluate the sums ∑ k |ν 1k|2, ∑ k |µ 1k ν 1k|2 and ∑ kl>k |µ 1k ν 1l+µ 1l ν 1k|2. The first sum

r=0sν1r+12=[s(L1)(1T2s)(1+T)]4.
(140)

r=0sμ1r+1ν1r+12={(1T2s)2+(L1)2[s2T2(1T2s)(1T2)
+T4(1T4s)(1T4)]}16.
(141)

For a long link, ∑ k |µ 1k ν 1k|2≈[s(L-1)2-1]=16. It is convenient to split the third sum into two parts. The first part

r=1sμ11ν1r+1+μ1r+1ν112=(L1)[s2Ts+1(1Ts)(1T)
+T2s+2(1T2s)(1T2)]4.
(142)

For a long link, ∑l>1|µ 11 ν 1l+µ 1l ν 11|2s(L-1)/4. The second part involves contributions of the form

r=q+1sμ1q+1ν1r+1+μ1r+1ν1q+12=(L1)2[(sq)2Ts+2q(1Tsq)(1T)
+T2s+42q(1T2s2q)(1T2)]4,
(143)

where 1≤qs-1. It is not difficult to sum these contributions. For a long link, ∑ k >1∑l>k |µ 1k ν 1l+µ 1l ν 1k|2s(s-1)(L-1)2=8. By combining the preceding results, one finds that

2kμ1kν1k2+kl>kμ1kν1l+μ1lν1k2{[1+s(L1)]22}8,
(144)

as stated in Eq. (106).

Acknowledgment

We acknowledge a useful discussion with M. V. Vasilyev.

References and links

1.

K. O. Hill, D. C. Johnson, B. S. Kawasaki, and R. I. MacDonald, “CW three-wave mixing in single-mode optical fibers,” J. Appl. Phys. 49, 5098–5106 (1978). [CrossRef]

2.

R. H. Stolen and J. E. Bjorkholm, “Parametric amplification and frequency conversion in optical fibers,” IEEE J. Quantum Electron. 18, 1062–1072 (1982). [CrossRef]

3.

J. Hansryd and P. A. Andrekson, “Broad-band continuous-wave pumped fiber optical parametric amplifier with 49-dB gain and wavelength-conversion efficiency,” IEEE Photon. Technol. Lett. 13, 194–191 (2001). [CrossRef]

4.

S. Radic, C. J. McKinstrie, R. M. Jopson, Q. Lin, and G. P. Agrawal, “Record performance of a parametric amplifier constructed with highly-nonlinear fiber,” Electron. Lett. 39, 838–839 (2003). [CrossRef]

5.

K. Inoue, “Tunable and selective wavelength conversion using fiber four-wave mixing with two pump lights,” IEEE Photon. Technol. Lett. 6, 1451–1453 (1994). [CrossRef]

6.

K. Uesaka, K. K. Y. Wong, M. E. Marhic, and L. G. Kazovsky, “Wavelength exchange in a highly nonlinear dispersion-shifted fiber: theory and experiments,” IEEE J. Sel. Top. Quantum Electron. 8560–568 (2002). [CrossRef]

7.

T. Tanemura, C. S. Goh, K. Kikuchi, and S. Y. Set, “Highly efficient arbitrary wavelength conversion within entire C-band based on nondegenerate fiber four-wave mixing,” IEEE Photon. Tech. Lett. 16, 551–553 (2004). [CrossRef]

8.

J. Hansryd, P. A. Andrekson, M. Westlund, J. Li, and P. O. Hedekvist, “Fiber-based optical parametric amplifiers and their applications,” IEEE J. Sel. Top. Quantum Electron. 8, 506–520 (2002). [CrossRef]

9.

S. Radic and C. J. McKinstrie, “Two-pump fiber parametric amplifiers,” Opt. Fiber Technol. 9, 7–23 (2003). [CrossRef]

10.

S. Radic and C. J. McKinstrie, “Optical parametric amplification and signal processing in highly-nonlinear fibers,” IEICE Trans. Electron. E88C, 859–869 (2005). [CrossRef]

11.

C. M. Caves, “Quantum limits on noise in linear amplifiers,” Phys. Rev. D 26, 1817–1839 (1982). [CrossRef]

12.

W. H. Louisell, Radiation and Noise in Quantum Electronics (McGraw-Hill, 1964).

13.

R. Loudon, The Quantum Theory of Light, 3rd Ed. (Oxford University Press, 2000).

14.

M. G. Raymer and M. Beck, “Experimental quantum state tomography of optical fields and ultrafast statistical sampling,” in Lecture Notes in Physics, Vol. 649, edited by M. Paris and J. Rehacek (Springer-Verlag, 2004), pp. 235–295.

15.

R. Loudon and P. L. Knight, “Squeezed light,” J. Mod. Opt. 34, 709–759 (1987). [CrossRef]

16.

C. J. McKinstrie, S. Radic, and M. G. Raymer, “Quantum noise properties of parametric amplifiers driven by two pump waves,” Opt. Express 12, 5037–5066 (2004). [CrossRef] [PubMed]

17.

C. J. McKinstrie, S. Radic, R. M. Jopson, and A. R. Chraplyvy, “Quantum noise limits on optical monitoring with parametric devices,” submitted to Opt. Commun.

18.

C. J. McKinstrie and S. Radic, “Phase-sensitive amplification in a fiber,” Opt. Express 12, 4973–4979 (2004). [CrossRef] [PubMed]

19.

C. J. McKinstrie, M. G. Raymer, S. Radic, and M. V. Vasilyev, “Quantum mechanics of phase-sensitive amplification in a fiber,” submitted to Opt. Commun.

20.

R. Loudon, “Theory of noise accumulation in linear optical-amplifier chains,” IEEE J. Quantum Electron. 21, 766–773 (1985). [CrossRef]

OCIS Codes
(060.2320) Fiber optics and optical communications : Fiber optics amplifiers and oscillators
(190.4410) Nonlinear optics : Nonlinear optics, parametric processes
(270.2500) Quantum optics : Fluctuations, relaxations, and noise

ToC Category:
Research Papers

History
Original Manuscript: May 16, 2005
Revised Manuscript: June 14, 2005
Published: June 27, 2005

Citation
C. McKinstrie, M. Yu, M. G. Raymer, and S. Radic, "Quantum noise properties of parametric processes," Opt. Express 13, 4986-5012 (2005)
http://www.opticsinfobase.org/oe/abstract.cfm?URI=oe-13-13-4986


Sort:  Journal  |  Reset  

References

  1. K. O. Hill, D. C. Johnson, B. S. Kawasaki and R. I. MacDonald, �??CW three-wave mixing in single-mode optical fibers,�?? J. Appl. Phys. 49, 5098�??5106 (1978). [CrossRef]
  2. R. H. Stolen and J. E. Bjorkholm, �??Parametric amplification and frequency conversion in optical fibers,�?? IEEE J. Quantum Electron. 18, 1062�??1072 (1982). [CrossRef]
  3. J. Hansryd and P. A. Andrekson, �??Broad-band continuous-wave pumped fiber optical parametric amplifier with 49-dB gain and wavelength-conversion efficiency,�?? IEEE Photon. Technol. Lett. 13, 194�??191 (2001). [CrossRef]
  4. S. Radic, C. J. McKinstrie, R. M. Jopson, Q. Lin and G. P. Agrawal, �??Record performance of a parametric amplifier constructed with highly-nonlinear fiber,�?? Electron. Lett. 39, 838�??839 (2003). [CrossRef]
  5. K. Inoue, �??Tunable and selective wavelength conversion using fiber four-wave mixing with two pump lights,�?? IEEE Photon. Technol. Lett. 6, 1451�??1453 (1994). [CrossRef]
  6. K. Uesaka, K. K. Y. Wong, M. E. Marhic and L. G. Kazovsky, �??Wavelength exchange in a highly nonlinear dispersion-shifted fiber: theory and experiments,�?? IEEE J. Sel. Top. Quantum Electron. 8 560�??568 (2002). [CrossRef]
  7. T. Tanemura, C. S. Goh, K. Kikuchi and S. Y. Set, �??Highly efficient arbitrary wavelength conversion within entire C-band based on nondegenerate fiber four-wave mixing,�?? IEEE Photon. Tech. Lett. 16, 551�??553 (2004). [CrossRef]
  8. J. Hansryd, P. A. Andrekson, M. Westlund, J. Li and P. O. Hedekvist, �??Fiber-based optical parametric amplifiers and their applications,�?? IEEE J. Sel. Top. Quantum Electron. 8, 506�??520 (2002). [CrossRef]
  9. S. Radic and C. J. McKinstrie, �??Two-pump fiber parametric amplifiers,�?? Opt. Fiber Technol. 9, 7�??23 (2003). [CrossRef]
  10. S. Radic and C. J. McKinstrie, �??Optical parametric amplification and signal processing in highly-nonlinear fibers,�?? IEICE Trans. Electron. E88C, 859�??869 (2005). [CrossRef]
  11. C. M. Caves, �??Quantum limits on noise in linear amplifiers,�?? Phys. Rev. D 26, 1817�??1839 (1982). [CrossRef]
  12. W. H. Louisell, Radiation and Noise in Quantum Electronics (McGraw-Hill, 1964).
  13. R. Loudon, The Quantum Theory of Light, 3rd Ed. (Oxford University Press, 2000).
  14. M. G. Raymer and M. Beck, �??Experimental quantum state tomography of optical fields and ultrafast statistical sampling,�?? in Lecture Notes in Physics, Vol. 649, edited by M. Paris and J. Rehacek (Springer-Verlag, 2004), pp. 235�??295.
  15. R. Loudon and P. L. Knight, �??Squeezed light,�?? J. Mod. Opt. 34, 709�??759 (1987). [CrossRef]
  16. C. J. McKinstrie, S. Radic and M. G. Raymer, �??Quantum noise properties of parametric amplifiers driven by two pump waves,�?? Opt. Express 12, 5037�??5066 (2004). [CrossRef] [PubMed]
  17. C. J. McKinstrie, S. Radic, R. M. Jopson and A. R. Chraplyvy, �??Quantum noise limits on optical monitoring with parametric devices,�?? submitted to Opt. Commun.
  18. C. J. McKinstrie and S. Radic, �??Phase-sensitive amplification in a fiber,�?? Opt. Express 12, 4973�??4979 (2004). [CrossRef] [PubMed]
  19. C. J. McKinstrie, M. G. Raymer, S. Radic and M. V. Vasilyev, �??Quantum mechanics of phase-sensitive amplification in a fiber,�?? submitted to Opt. Commun.
  20. R. Loudon, �??Theory of noise accumulation in linear optical-amplifier chains,�?? IEEE J. Quantum Electron. 21, 766�??773 (1985). [CrossRef]

Cited By

Alert me when this paper is cited

OSA is able to provide readers links to articles that cite this paper by participating in CrossRef's Cited-By Linking service. CrossRef includes content from more than 3000 publishers and societies. In addition to listing OSA journal articles that cite this paper, citing articles from other participating publishers will also be listed.


« Previous Article  |  Next Article »

OSA is a member of CrossRef.

CrossCheck Deposited