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Optics Express

  • Editor: C. Martijn de Sterke
  • Vol. 15, Iss. 25 — Dec. 10, 2007
  • pp: 17151–17162

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Flat-top surface plasmon-polariton modes guided by double-electrode structures

Jaewoong Yoon, Seok Ho Song, and Suntak Park  »View Author Affiliations


Optics Express, Vol. 15, Issue 25, pp. 17151-17162 (2007)
http://dx.doi.org/10.1364/OE.15.017151


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Abstract

We characterize the frequency dependence of symmetrically-coupled long-range surface plasmon-polaritons (sc-LRSPPs) excited on double-electrode slab waveguides composed of five layers of insulator(I) and metal(M) stacked in order of IMIMI. When the core insulator has a refractive-index larger than the cladding ones, there is no cut-off core-thickness(D) for sc-LRSPP modes in all frequency range likely for modes in a conventional dielectric slab waveguide. At a specific frequency of ωc which depends on the index difference of insulator layers and the thickness of metal, the sc-LRSPP modes are non-dispersive at all for change in D. Furthermore, regardless of D alteration, the modes at ω=ωc consistently maintain a perfect flat-top profile in the core region and identical decay tails in the cladding. The sc-LRSPP modes with these prominent characteristics may excite an active medium sandwiched in between the metal layers very uniformly, therefore it will be interesting to implement such a non-dispersive flat-top mode for nonlinear applications of SPP waveguides.

© 2007 Optical Society of America

1. Introduction

Surface plasmon-polaritons (SPPs) are surface localized waves propagating on an interface between a metal and a dielectric. Over a frequency band in which the dielectric constant of metal is less than minus of that of adjacent dielectric, SPPs are excited by coupling between collective oscillations of free electrons and evanescent electromagnetic (EM) waves [1

H. Raether, Surface plasmons on Smooth and Rough Surfaces and on Gratings , (Springer-Verlag, Berlin, 1988).

,2

W. L. Barnes, A. Dereux, and T. W. Ebbesen, (Insight review articles) “Surface plasmon subwavelength optics,” Nature 424, 824–830 (2003). [CrossRef] [PubMed]

]. This resonant coupling gives SPPs the peculiar properties of surface localizations and field enhancements, which make a lightwave be able to interact strongly with nanoscopic structures by mediating them. For these natures, SPPs have been widely studied since the first optical observation in the anomalous diffraction from a metallic grating by Wood [3

R. W. Wood, “On a remarkable case of uneven distribution of light in a diffraction grating spectrum,” Phil. Mag. 4, 396 (1902).

,4

R. W. Wood, “Anomalous diffraction gratings,” Phys. Rev. 48, 928–936 (1935). [CrossRef]

] and its causal explanation by Fano [5

U. Fano, “The theory of anomalous diffraction gratings and of quasi-stationary waves on metallic surfaces (Sommerfeld’s waves),” J. Opt. Soc. Am. 31, 213–222 (1941). [CrossRef]

]. Applications of SPPs are ranging from colored glasses [6

S. Linden, J. Kuhl, and H. Giessen, “Controlling the interaction between light and gold nano particles: Selective suppression of extinction,” Phys. Rev. Lett. 86, 4688 (2001). [CrossRef] [PubMed]

] or attenuated total reflection (ATR) based devices [7

E. Kretchmann and H. Raether, “Radiative decay of nonradiative surface plasmons excited by light,” Z. Naturkorsch. A 23, 2135–2136 (1968).

–9

J. Homola, S. S. Yee, and G. Gauglitz, “Surface plasmon resonance sensors: review,” Sensors Actuat. B 54, 3–15 (1999). [CrossRef]

] to even potentials for merging photonic and electronic integrated circuits recently [2

W. L. Barnes, A. Dereux, and T. W. Ebbesen, (Insight review articles) “Surface plasmon subwavelength optics,” Nature 424, 824–830 (2003). [CrossRef] [PubMed]

,10

E. Ozbay, (Review) “Plasmonics: Merging photonics and electronics at nanoscale dimensions,” Science 311, 189–193 (2006). [CrossRef] [PubMed]

–13

J. R. Krenn and J.-C. Weeber, “Surface plasmon polaritons in metal stripes and wires,” Phil. Trans. R. Soc. Lond. A 362, 739–756 (2004). [CrossRef]

].

One of the active fields regarding SPPs is applications of long-range SPPs (LRSPPs). LRSPPs are supported by anti-symmetric charge coupling of SPPs on two surfaces of a thin metal film of which thickness is comparable to or less than the penetration depth of EM wave. For its small propagation constant and nearly transversal field components, internal loss (mainly ohmic loss in the metal) is small and direct end-fire coupling with any fundamental mode of a conventional dielectric based waveguide is very efficient [1

H. Raether, Surface plasmons on Smooth and Rough Surfaces and on Gratings , (Springer-Verlag, Berlin, 1988).

,14

D. Sarid, “Long-range surface-plasma waves on very thin metal films,” Phys, Rev. Lett. 47, 1927–1930 (1981). [CrossRef]

,15

P. Berini, “Plasmon-polariton waves guided by thin lossy metal films of finite width: Bounded modes of symmetric structures,” Phys. Rev. B 61, 10484 (2000). [CrossRef]

]. Though LRSPPs are not so confined modes and the loss is still larger than dielectric waveguides, high cladding sensitivity and parallelism of optical and electrical signals make them useful for integrated optical devices. In addition, LRSPP waveguides consisting of about 20 nm thick and a few µm wide metal strips are much easier to be fabricated by conventional lithography technique than index-guiding dielectric waveguides which require a wavelength scale depth in index steps. Many integrated passive and active optical devices based on LRSPPs such as channel waveguides [16

T. Nikolajsen, K. Leosson, I. Salakhutdinov, and S. I. Bozhevolnyi, “Polymer-based surface-plasmon-polariton stripe waveguides at telecommunication wavelengths,” Appl. Phys. Lett. 82, 668–670 (2003). [CrossRef]

,17

P. Berini, R. Charbonneau, N. Lahoud, and G. Mattiussi, “Characterization of long-range surface-plasmon-polariton waveguides,” J. Appl. Phys. 98, Art. No. 043109 (2005). [CrossRef]

], thermo-optic modulators [18

T. Nikolajsen, K. Leosson, and S. I. Bozhevolnyi, “In-line extinction modulator based on long-range surface plasmon polaritons,” Opt. Commun. 244, 455–459 (2005). [CrossRef]

–20

G. Gagnon, N. Lahoud, G. A. Mattiussi, and P. Berini, “Thermally activated variable attenuation of long-range surface plasmon-polariton waves,” J. Lightwave Technol. 24, 4391–4402 (2006). [CrossRef]

], directional couplers [21

A. Boltasseva, T. Nikolajsen, K. Leosson, K. Kjaer, M. S. Larsen, and S. I. Bozhevolnyi, “Integrated optical components utilizing long-range surface plasmon polaritons,” J. Lightwave technol. 23, 413–422 (2005). [CrossRef]

–23

R. Charbonneau, C. Scales, I. Breukelaar, S. Fafard, N. Lahoud, G. Mattiussi, and P. Berini, “Passive integrated optics elements based on long-range surface plasmon polaritons,” J. Lightwave Technol. 24, 477–494 (2006). [CrossRef]

], and Bragg grating filters [24

A. Boltasseva, S. I. Bozhevolnyi, T. Søndergaard, T. Nikolajsen, and K. Leosson, “Compact Z-add-drop wavelength filters for long-range surface plasmon polaritons,” Opt. Express 13, 4237–4243 (2005). [CrossRef] [PubMed]

,25

S. J. Charbonneau, R. Charbonneau, N. Lahoud, G. A. Mattuissi, and P. Berini, “Bragg gratings based on long-range surface plasmon-polariton waveguides: Comparison of theory and experiment,” IEEE J. Quantum Electron. 41, 1480–1491 (2005). [CrossRef]

] were reported recently in this context.

A double-electrode structure which consists of two metallic thin film had been reported as a possible waveguide structure supporting LRSPPs quite long time ago [26

G. I. Stegeman and J. J. Burke, “Long-range surface-plasmons in electrode structures,” Appl. Phys. Lett. 43, 221–223 (1983). [CrossRef]

]. Stegeman et al pointed out that LRSPPs on a double-electrode waveguide can be controlled more actively by using electro- or acousto-optic materials as a central dielectric medium because the pair of the metal film itself offers to supply DC electric field in the core dielectric medium. This structure has some other advantages over single-film LRSPP waveguides. As any homogeneous change in the core dielectric material does not break vertical symmetry of the structure, LRSPPs exist over much broader range of index contrast between the core and the cladding dielectric [26

G. I. Stegeman and J. J. Burke, “Long-range surface-plasmons in electrode structures,” Appl. Phys. Lett. 43, 221–223 (1983). [CrossRef]

]. Therefore, the structure does not require a nearly free standing metal film for LRSPP based fluidic sensors, and it can include dielectric grating or photonic crystal structures in the core dielectric medium. In spite of those advantages, little attention has been paid to a double-electrode LRSPP waveguide. Dispersion relations and attenuation properties of LRSPPs excited on a double-electrode waveguide had been reported [26

G. I. Stegeman and J. J. Burke, “Long-range surface-plasmons in electrode structures,” Appl. Phys. Lett. 43, 221–223 (1983). [CrossRef]

, 27

E. N. Economou, “Surface plasmons in thin films,” Phys. Rev. 182, 539–554 (1969). [CrossRef]

], but decisive questions for its practical applicability considering dependence of propagation lengths and field identities on operation frequency have not been addressed so far.

In this paper, we study frequency dispersive characteristics of LRSPPs on double-electrode waveguides. Dispersion curves and corresponding field identities of the modes are analyzed according to the structural parameters of core and cladding dielectrics. The analysis allows us to describe double-electrode LRSPPs in a general manner with the help of definition of a characteristic frequency by which different core-thickness dependencies are classified. Several interesting properties such as cut-off core-thickness at the vicinity of which the attenuation is largely reduced without any need of thinning metallic films, transiently saturated attenuation which can be used as a switching operation point, and the thickness-dispersionless flat-top LRSPP which can provide efficient adiabatic mode scaling are discussed on this basis. In section 2, dispersion relation of double-electrode waveguide structures is briefly derived. Dispersion curves in terms of frequency and effective-index of LRSPP modes are presented in Section 3, where dependence of the dispersion relation on the core-thickness is discussed for both low-index-core and high-index-core structures. The characteristic frequency that offers a criterion classifying the characteristic groups of LRSPP modes is described in Section 4. Field identities and attenuation properties at relative frequencies to ωc are investigated in Section 5. Finally we conclude our analysis on double-electrode waveguide structures in Section 6.

Fig. 1. Schematic of a double-electrode slab waveguide structure and the shape of magnetic field profile for a symmetrically coupled LRSPP.

2. Dispersion relation of double-electrode waveguides

A double-electrode waveguide considered here is illustrated in Fig. 1. It consists of two identical metal slabs with a dielectric constant ε2 surrounded by core (ε1 ) and cladding (ε3 ) dielectrics. Thickness of the core dielectric and the metal film is D and t, respectively. In frequency domain, the magnetic field of a transverse magnetic (TM) polarized mode with propagation constant β in this structure can be written in general as

H= H0f (y)exp (iβx) ez,
(1)

where

f (y)= { cosh ( α1y) or sinh ( α1y) ( 0≤ y≤D⁄2) Aexp ( α2 [ y−D⁄2])+Bexp (− α2 [ y−D⁄2]) ( D⁄2≤ y≤ t+D⁄2) Cexp (− α3 [ y−D⁄ 2−t]) ( t+ D⁄2≤y)
(2)

in the region y≥0. The cosh(α1y ) or sinh(α1y ) is taken for a symmetric or an anti-symmetric mode respectively. The field in the region y≤0 is also provided by continuation of Eq. (2), and the electric field is given by E=-∇×H/(iωεm ) for m=1, 2, or 3. The decay constant in each layer is given by

αm= ( β2− εm k02) 1⁄2,m=1,2, or 3.
(3)

Requiring continuity of the tangential fields (Hz and Ex ) at the interfaces leads to a dispersion relation and the amplitudes of a symmetric mode, A, B, and C in Eq. (2), as follows.

α2 α3 ε2 ε3+ α1 α2 ε1 ε2tanh ( α1D⁄2)+ ( α2 ε2)2tanh ( α2t)+ α3 α1 ε3 ε1tanh ( α1D⁄2)tanh ( α2t)=0
(4)
{ A= 12 [ cosh ( α1D⁄2)+ α1⁄ ε1 α2⁄ ε2sinh ( α1D⁄2)] B= 12 [ cosh ( α1D⁄2)− α1⁄ ε1 α2⁄ ε2sinh ( α1D⁄2)] C= [ cosh ( α1D⁄2)cosh ( α2t)+ α1⁄ ε1 α2⁄ ε2sinh ( α1D⁄2)sinh ( α2t)]
(5)

Expressions for an anti-symmetric mode can be obtained by exchanging cosh and sinh to each other. The dispersion relation in Eq. (4) gives a complex propagation constant of β=βr+iβi . Frequency dependent characteristics of βr provide a dispersion curve according to D, and 1/(2βi ) defines propagation length where the mode intensity is decayed down to its 1/e value after propagation.

It is known that four modal solutions exist implicitly in Eq. (4) as SPP modes for a double-electrode structure [26

G. I. Stegeman and J. J. Burke, “Long-range surface-plasmons in electrode structures,” Appl. Phys. Lett. 43, 221–223 (1983). [CrossRef]

,27

E. N. Economou, “Surface plasmons in thin films,” Phys. Rev. 182, 539–554 (1969). [CrossRef]

]. Each of them represents a combination out of symmetrically or anti-symmetrically coupled (sc- or ac-) long-range SPPs (LRSPPs) or short-range SPPs (SRSPPs). Internal loss is smaller in long-range SPP modes while larger in short-range SPP modes since they possess a node in the metal slabs. Each of the long-range and short-range SPPs splits again into two separate modes according to their symmetry referenced at the center of the core dielectric. Only a symmetrically-coupled long-range SPP, sc-LRSPP, mode whose magnetic field has a profile depicted schematically in Fig. 1 will be considered hereafter, because an anti-symmetrically coupled long-range SPP may hardly be excited by direct end-fire coupling and even disappears when the core thickness is less than about the decay length of SPPs excited on a single-electrode waveguide [26

G. I. Stegeman and J. J. Burke, “Long-range surface-plasmons in electrode structures,” Appl. Phys. Lett. 43, 221–223 (1983). [CrossRef]

].

Complex β which satisfies Eq. (4) is found by 2 stage processes. On the first stage, an approximate solution is given by observing values of left-hand side of Eq. (4). Reciprocals of absolute square values of the left-hand side of Eq. (4) are evaluated along real β-axis within a specified domain of β. A range ε 3 1/2 k0 <β<2ε 3 1/2 k 0 was enough to completely contain the sc-LRSPP dispersion curve for an arbitrary core thickness over a frequency domain from DC to visible light. The reciprocal of absolute square value of the equation shows series Lorentzian-shaped peaks centered at Re{β sc-LRSPP} and Re{β sc-SRSPP}. The peak center position (β0 ) closest to ε 3 1/2 k0 among them is recognized as an initial guess for βr of the sc-LRSPP. Its full-width at half-maximum (Δβ) is assigned as an approximate value of 2βi . On the second stage, Newton method starting at β (0)=β 0+iΔβ/2 is applied to find the exact complex β for the sc-LRSPP until the propagation constant converges within |β((n+1)-β( (n) |/k 0=±1.1×10-16 during consecutive iterations. As βi/βr is an order of 10-3 or less (β is dominantly real), the first stage gives a well defined initial guess and provides a good repeatability in finding roots.

3. Symmetrically-coupled long-range surface plasmon-polaritons

Two different cases of low-index-core and high-index-core structures are analyzed to find out global features of sc-LRSPPs. Let’s specify, for simplicity, the metal slabs by a 20 nm-thick gold film and the refractive index of the core (cladding) dielectric by 1.45 (1.47) for the low-index-core structure and by 1.47 (1.45) for the high-index-core structure, as shown in the insets of Fig. 2. Dispersion curves calculated by Eq. (4) are shown in Fig. 2 for the two core structures. The effective index of a sc-LRSPP mode is defined as a relative propagation constant of neff =βr/k0 , and the frequency is normalized by the frequency of an electromagnetic wave whose vacuum wavelength is 1 µm. A Drude model fitted to give ε 2=-118+11.58i at 1550 nm vacuum wavelength is used for the frequency dependent dielectric constant of Au [28

E. D. Palik, Handbook of Optical Constants of Solids II , (Academic Press, San Diego, 1998).

].

Figures 2(a) and 2(b) show frequency dispersive characteristics of the effective indices for the sc-LRSPP modes exited at the two double-electrode waveguide structures with low-index-core and high-index-core, respectively. The dispersion curves exist only in the shadow regions as D increases from 0 µm to infinity, and those depicted in between the two asymptotic limits are of the finite core-thickness ranging from 0.2 µm to 6.0 µm in 0.2 µm steps. It is worth discussing first the two limits of no core dielectric (D=0 µm) and infinitely thick core dielectric (D→∞). The dispersion curves and modal properties for any other finite cores will be addressed in between these two limits as shown in Fig. 2. For the limit case when D=0 µm, the dispersion curves exist over the continuous range starting from the zero frequency for both core-index structures. This no-core limit is the same as the dispersion of LRSPP modes for a single-electrode waveguide with a metal thickness of 2t (40 nm). On the other hand, the dispersion curves when D→∞ have a characteristic frequency ωc at the point of 1.47 effective index. In the frequency range smaller than ωc there is no LRSPP mode for the infinite core thickness. Since when D→∞ there is no coupling between the modes on the two metal waveguides, the dispersion curves shown above the ωc are the same as the dispersion of a asymmetric single-electrode waveguide composed by a metal film with thickness of t (20 nm) and two different surrounding dielectrics with n=1.45 and n=1.47. In the case of the 20 nm-thick Au film sandwiched by two dielectrics with the refractive indices of 1.45 and 1.47, ωc is 1.09×2πc/µm and the corresponding vacuum wavelength is 917.08 nm.

For a finite core-thickness in the low-index-core structure shown in Fig. 2(a), there is no low frequency cut-off in the dispersion curve as D increases up to 1.0 µm. For a core-thickness larger than 1.0 µm, on the other hand, low-frequency cut-off appears and it approaches ωc as D increases. Therefore the core-thickness dependent characteristics of sc-LRSPP modes is quite different according to the relative position of the frequency to ωc . For a fixed frequency lower than ωc , as D gets larger, the effective index decreases down to the cladding index of n 3 (1.47) as D approaches a particular value, Dcut-off, and the sc-LRSPP modes disappear when D>Dcut-off . That is, there is a range of the core thickness that supports sc-LRSPPs when ω<ωc . This behavior of the effective index is shown in Fig 2(c). Dashed and dash-dotted line represents D-dependent effective index at two different frequencies below ωc . Corresponding vacuum wavelength is 1550(ω 1) and 1100(ω 2) nm, respectively. Please note that grey lines below 1.47 indicate not true solution but initial guesses given by peak positions of reciprocal value of the dispersion equation. There is no β satisfying Eq. (4) below effective index of 1.47. It is confirmed that the effective index decreases for increasing D and finally disappear for D>Dcut-off. Dcut-off is 1.340 µm for ω 1 and 1.688 µm for ω 2. For a core thickness just below Dcut-off , the mode size diverges to infinity since the decay constant in the cladding given by α 3=[β2-n3 2k02]1/2 is about to vanish and therefore the decay length of the evanescent tail (1/α 3) stretched into the cladding diverges to infinity. The energy dissipated as ohmic loss in the metal will vanish too as shown in Fig 2(d). Therefore, it is expected that the propagation length will be largely extended just before the mode cut-off. Dcut-off becomes larger for a higher frequency and infinite when ω=ωc . For ω>ωc there is no cut-off core thickness and therefore no drastic extension in the propagation length is expected over the frequency range higher than ωc .

Fig. 2. The dispersion curves of sc-LRSPPs for two different cases of (a) low index core (n1=1.45, n 3=1.47) and (b) high index core (n1=1.47, n3=1.45). Two asymptotic limits of D=0 µm and D=∞ are indicated by two thick curves on the boundaries of grey regions, and the dispersion curves in the grey region are of the core thicknesses ranging from 0.2 µm to 6.0 µm in 0.2 µm step. Please note that the core is thicker as the curve approaches the boundary of the grey region marked by ‘D=∞’. (c) and (d) shows thickness dispersive characteristics of effective index and βi for several frequencies below ωc , respectively. Relative locations in the dispersion diagram for ω 1 and ω 2 are indicated by horizontal lines in (a).

On the other case of the high-index-core structure, frequency dependence of the sc-LRSPP modes is quite interesting as shown in Fig. 2(b). All curves are crossing at a single position at (n 1,ωc ) regardless of the value of D. When ω=ωc the propagation constant of sc-LRSPP mode is non-dispersive on D. Any cut-off core thickness does not exist over the full frequency range, so the internal loss of the sc-LRSPP modes never decreases extremely low. For ω <ωc the effective index has a value less than n 1 (1.47) and gradually approaches n1 as D increases, while for ω >ωc dependence of the dispersion relation on D is similar to the low-index-core case. The sc-LRSPP mode with a larger core thickness reduces to a fundamental mode of dielectric slab waveguide which consists of the same core and cladding dielectrics without metal. A physical origin of existence of the crossing point at (n 1,ωc ) in the high-index-core structure can be clearly found by requiring Eq. (4) to be specified at the condition that β=n1k0 and α 1=0. Under this specific condition, the dispersion relation is reduced to (α3/ε3 )+(α2/ε2 ) tanh(α2t)=0, and therefore it has no dependence on D. It can be deduced that eigen frequencies of the sc-LRSPP modes which have the effective index equal to the core index must keep in constant to be ωc even for core-thickness variation.

Now we would like to summarize the frequency-dependent characteristics of sc-LRSPP modes excited on double-electrode structures as follows: In low-index-core case shown in Fig. 2(a), a cut-off core thickness exists for sc-LRSPP modes at a frequency range less than the characteristic frequency ωc and mode size and propagation length become extremely extended just before the cut-off. For ω >ωc , on the other hand, a sc-LRSPP mode can always be supported for arbitrary core thickness without a drastic extension of its mode size and propagation length. In low-index-core case shown in Fig. 2(b), when ω<ωc sc-LRSPP modes approach a fundamental mode of dielectric slab waveguide gradually from a single-electrode LRSPP mode as D increases. At ω=ωc the propagation constants of sc-LRSPP modes are non-dispersive and equal to n 1 k 0 even for core-thickness variation. For ω>ωc , the frequency-dependent characteristics are the same as the low-index case.

4. The characteristic frequency

The characteristic frequency ωc can be derived from the dispersion relation when propagation constant has no dependence on D, (α3/ε3 )+(α2/ε2 ) tanh(α2t)=0, as follow.

ωc= ct 1 [ ε1− ε2 ( ωc)] 1⁄2 tanh −1 (− ε2 ( ωc) ε3 [ ε1− ε3 ε1− ε2 ( ωc)] 1⁄2)
(6)

To extract the value of ωc in terms of the three dielectric constants and the metal thickness is not straightforward, but it is plausible to estimate its dependence on the index contrast, Δn=n3-n1 , between the dielectric layers. If Δn=0(viz. ε1-ε3 =0), ωc =0 obviously. For a non-zero or even a large Δn, intuitively ωc can be estimated from the dispersion diagrams in Fig. 2(b). In fact, the reduced equation of (α3/ε3 )+(α2/ε2 ) tanh(α2t)=0 is exactly the same as the dispersion relation of LRSPPs excited on a single-electrode waveguide consisting of a single metal slab with thickness of 2t surrounded by dielectric with ε3. ωc is the frequency of the LRSPP mode on this single-electrode waveguide when the relation β=n 1 k 0 satisfied.

Fig. 3. Dependences of the characteristic frequency on the index difference for several refractive indices of the cladding (a) and some thicknesses of the metal slab (b). The Au thickness is fixed at 20 nm for (a), and the refractive index of the cladding is fixed at 1.45 for (b) respectively.

Therefore, for the structures considered in Fig. 2, ωc is a point corresponding to the effective index of n 1. If n 1 increases, ωc increases along the curve for D=0 µm. For a large Δn, ωc approaches a cut-off frequency of the single-electrode LRSPP, that is ωc →ωp /(1+ε3 )1/2.

Figure 3 shows dependence of ωc on the index contrast Δn and the metal thickness t. In Fig. 3(a), the cladding index n 3 is chosen from some typical dielectric materials like silica (1.45), LiNbO3 (2.2142), and silicon (3.4764) taken in the Ref. 40 by interpolating at λ 0=1550 nm, while the metal thickness is fixed at 20 nm. It can be confirmed that ωc converges to ωp/(1+ε3 )1/2 for a large index contrast. In the order of n 3=1.0, 1.33, 1.45, 2.2142, and 3.4764, the values of ωp /(1+ε3 )1/2 normalized by 2πc/µm are 5.00, 4.25, 4.01, 2.91, and 1.95, respectively. In the same order of n 3, Δn that gives ωc corresponding to the vacuum wavelength of 1550 nm is 2.14×10-3, 5.09×10-3, 6.62×10-3, 2.44×10-2, and 1.30×10-1, respectively. For n 3=1.45, the ωc dependence on the metal thickness is shown in Fig. 3(b). As Δn increases, ωc converges to a constant value of 6.62×10-3 even for the different thickness, but ωc grows more rapidly for a smaller t. It is confirmed that ωc is tunable over broad spectrum from an optical communication to whole visible frequency range with acceptable index differences of 10-3~1.

5. Propagation lengths and field profiles

Figures 4(a) and 5(a) show propagation length defined by 1/(2βi ) for sc-LRSPP modes excited on the two double-electrode structures with low-index core and high-index core, respectively. D varies from 0 µm to 8 µm. Three representative vacuum wavelengths (λ 0) of 667 nm, 917 nm, and 1550 nm are selected to compare the propagation lengths for three different frequency regions of ω<ωc , ω=ωc (=3.27×1014 rad./s), ω>ωc , respectively. In case of low-index core shown in Fig. 4(a), frequency characteristics of sc-LRSPP propagation length dependent on D variation are clearly recognizable with the three black line curves. At λ0 =1550 nm (ω < ωc , dashed black line), the propagation length increases exponentially for a small core thickness up to 0.7 µm before the transient saturation at the vicinity of 1 µm, and it gradually diverges without any supported sc-LRSPP mode after 1.33 µm. The behaviors of the exponential increase and the transient saturation are also seen at λ 0=917 nm (ω=ωc , dash-dotted black line) bellow the 1.5 µm core-thickness. The two grey curves near the solid black line of 917 nm represent those for the frequencies adjacent to ωc , for instance, ωc -0.17×106 rad./s for the upper grey and ωc +2.07×106 rad./s for the lower grey line. At λ 0=667 nm (ω>ωc ), on the other hand, the propagation length keep in constant for large D variations. It is noted that, at ω=ωc , the propagation length does not go to infinity abruptly after the transient saturation but increases exponentially and that the propagation behavior suffers from a sudden divergence or a bound limit even for a small amount of frequency deviation from ωc .

Fig. 4. (a). Dependences of the propagation lengths of sc-LRSPPs on the core thickness for the case of low index core at several wavelengths. The vacuum wavelengths are selected as representatives for ω<ωc (dashed line), ω=ωc (black solid line) and ω>ωc (dash-dotted line). Each of the upper and the lower grey solid curve represents just below and over the characteristic frequency respectively, and the corresponding differences from ωc are -0.17 and +2.07×106 rad./s. (b) Field profiles (Hz ) of a sc-LRSPP at ω=ωc for the case of low index core. The inset shows the profiles normalized by its value at the core-metal interface in the metal film. In the inset, grey region indicates the metal film.

A reason exhibiting the transient saturation near the core thickness of about wavelength scale can be found from transition property of the mode profiles as D varies. Figure 4(b) shows the normalized Hz components of sc-LRSPP modes when D=0.3, 1.0, and 4.0 µm, where the surface normal position at 0 µm means the center of the core dielectric and those at the peaks indicate the positions of the metal slabs. The inset in Fig. 4(b) is the magnified Hz profiles around the 20 nm-thick metal embedded in between the core (n 1) and the cladding (n 3). All the mode profiles reveal necessarily exponential decay in the cladding and hyperbolic-cosine distribution in the core, but the ratio of the field amplitudes at the two metal-dielectric interfaces is quite different with each other. At D=0.3 µm, before the transient saturation in propagation length, the field amplitude is smaller at the metal-core interface and it grows up inside the metal layer as approaching the metal-cladding interface. At D=1.0 µm within the transient saturation region or at D=4.0 µm after it, on the other hand, the field amplitude, decreases down toward the metal-cladding interface. This difference in the field profiles can be understood by a transition property of the mode profiles between two limiting cases of D=0 and D→∞: When the core thickness shrinks to be zero the field profiles on two metal slabs combine together to make a single hyperbolic-cosine form, therefore the field amplitudes on both sides of the metal-dielectric interfaces become higher than that in the middle of the metal layer. If the core thickness is large enough not to allow any field coupling between the two metals, the field in each metal slab has a larger amplitude on the metal boundary facing the dielectric with a lower refractive index since the evanescent tail of the field profile is stretched further into the lower dielectric.

In case of the high-index core shown in Fig. 5, change in the propagation length as D varies is moderate with no drastic increase for all three wavelengths. (Note that the vertical scale is linear, not logaritmic as in Fig. 4(a)). For λ 0=1550 nm the propagation length decreases gradually down to a minimum at D=3 µm before its increase. The normalized Hz profiles for D=0.3, 3.0, and 8.0 µm depicted in Fig. 5(b) imply that the energy portion localized in the core region becomes larger as increasing D and the mode approaches to a fundamental mode of dielectric slab waveguides. Also, the field amplitudes inside the metal layer always grow up as approaching the metal-cladding interface as shown in the inset of Fig. 5(b).

Fig. 5. (a). Dependences of the propagation lengths of sc-LRSPPs on the core thickness for the case of high index core at several wavelengths. The vacuum wavelengths are selected as representatives for ω<ωc (dotted line), ω=ωc (solid line) and ω>ωc (dash-dotted line). Please note that, differently from Fig. 4(a), the vertical axis is not logarithmic but linear scale. (b), (c), and (d) shows the field profiles (Hz) of sc-LRSPPs for several core thicknesses at ω<ωc , ω=ωc , and ω>ωc respectively. The inset in each figure shows the profiles normalized by its value at the core-metal interface in the metal film (grey region).

For λ 0=917 nm (ω=ωc ), dependence of the propagation length on D and evolution of the field profiles are quite interesting as depicted in Figs. 5(a) and 5(c), respectively. The propagation length is linearly proportional to D. Regardless of the core thickness, the field amplitude is uniform over the whole core region and the normalized field profiles around the metal layers are exactly matched with each other as shown in the inset of Fig. 5(c). These distinctive characteristics at ω=ωc are caused by the fact that β=n 1 k 0 thus α 1=0 for arbitrary core thickness. The non-dispersive property of the propagation constants on D also insists that α 2 and α 3 must be constant, therefore, not only the decay lengths to the core and cladding dielectrics but also the amplitudes of the exponents given in Eq. (5) should be constant. It must be emphasized that this particular property is very desirable for adiabatic coupling between optical modes with different lateral sizes via waveguide tapering. Adiabatic coupling is reasonable under the condition that the eikonal parameter defined by tan(ϕ)[d(1/βr )/dD] should be much less than 1, where ϕ is a taper angle [29

M. I. Stockman, “Nanofocusing of optical energy in tapered plasmonic waveguides,” Phys. Rev. Lett. 93, Art. No. 137404 (2004). [CrossRef] [PubMed]

]. The eikonal parameter is zero for sc-LRSPP modes with the characteristic frequency, resulting that a very large tapering angle can be acceptable for an efficient mode coupling. Moreover, the flat-top profiles of the field amplitudes in the core are sustained even for a large core-thickness variation. This may offer a noble method for flat-top beam shaping of light radiated from a conventional waveguide or a point-like source.

Finally over a higher frequency range of ω>ωc , core-thickness dependence of the propagation length in Fig. 5(a) and the mode profiles in Fig. 5(d) are not so different from those of the low-index-core case. The modes converge to a decoupled LRSPP mode from a sc-LRSPP as increasing D with no distinct feature in between.

It may be worth considering whether such a crossing in dispersion curves as shown in Fig. 2(b) also takes place in a two dimensional guiding structure, like a cylindrical plasmonic waveguide consisting of a metal coated high-index dielectric wire surrounded by a low-index cladding [30

U. Schröter and A. Dereux, “Surface plasmon polaritons on metal cylinders with dielectric core,” Phys. Rev. B 64, Art. No. 125420 (2001). [CrossRef]

]. Actually the SPP mode represented by n=1 in a higher branch of dispersion curve of the cylindrical plasmonic waveguide, where n is the number of azimuthal oscillation, also has a crossing point near the core light line. According to Ref. 30, dispersion curves for higher branch of n=1 modes cross core light line and curves for different core diameter intersect with each other. Therefore, it can be concluded that there exists flat-top modes (α 1=0) and nearly non-dispersive characteristics on core diameter. But unfortunately, we have found that the crossing point does not always correspond to the core light line after an intuitive consideration as follow: Noted that one of the physical origins of the non-dispersive characteristic at ω=ωc results from the separable property of the exponential functions in Eqs. (4) and (5) so as to satisfy exp[±α 2(D+t)]=exp(±α2D)exp(±α2t). These separable functions guarantee to eliminate the term exp(±α2D) in Eqs. (4) and (5), and only the exponents having ±α1D argument among the D dependent terms survive before they disappears when α 1=0 at ω=ωc . However, such elimination is not possible in a cylindrical plasmonic waveguide because its mode expression does not consist of exponential functions any more but modified Bessel functions of second kind. Therefore, a flat-top mode exists in a cylindrical plasmonic waveguide, but it does not always have non-dispersive characteristic on core diameter. Though the two noble properties do not always coincide with each other, it will be interesting to find out other 2-dimensional structures that support efficient flat-top collimation or coupling between optical source and µm-scale waveguide.

6. Conclusion

For double-electrode plasmonic waveguide structures, modal properties of the sc-LRSPPs have been described comprehensively by investigating frequency dependence of the dispersion relation and the mode profiles consistently. We have found out that the sc-LRSPP modes excited on a double-electrode plasmonic waveguide can be classified by four groups of distinctive characters according to their dependence on the core thickness D. For the low-index-core structure, the propagation length can be largely extended at a particular core thickness of wavelength scale at a frequency range lower than the characteristic frequency ωc which depends on the index difference in the core-cladding layers and the thickness of the metal. The characteristic of drastic increase in the propagation length may be used not only for refractrometric sensors or non-linear ATR devices but also variable optical attenuators by incorporating media for active index modulation as a core dielectric [19

S. Park and S. H. Song, “Polymeric optical attenuator based on long range surface plasmon polaritons,” Electron. Lett. 42, 402–404 (2006). [CrossRef]

]. For a frequency range higher than ωc , the sc-LRSPP mode converts its modal property moderately from symmetrically coupled to decoupled as D increases. For the high-index-core structure, on the other hand, there is no cut-off core thickness in overall frequency range. For ω<ωc the sc-LRSPPs with a large D converge to a mode of conventional dielectric slab waveguides, but at ω=ωc the sc-LRSPP modes are completely non-dispersive for change in D. Regardless of D alteration, the modes at ω=ωc consistently maintain a perfect flat-top profile in the core region and identical decay tails in the cladding. 2-dimensional extension of this prominent characteristic may provide us a novel means for uniform dimension-scaling and flat-top profile-shaping of an optical mode tightly guided by plasmonic waveguides. Thus it will be worth to find out conditions for flat-top modes in a cylindrical waveguide with metal coated dielectric core. The flat-top sc-LRSPP modes may excite an active medium sandwiched in between the metal layers very uniformly, therefore it will be interesting to implement such a non-dispersive flat-top mode for nonlinear applications of SPP waveguides.

Acknowledgments

This work was supported by an ETRI (Electronics and Telecommunications Research Institute) of Korea committed project (Grant No. 1010-2006-0111).

References and links

1.

H. Raether, Surface plasmons on Smooth and Rough Surfaces and on Gratings , (Springer-Verlag, Berlin, 1988).

2.

W. L. Barnes, A. Dereux, and T. W. Ebbesen, (Insight review articles) “Surface plasmon subwavelength optics,” Nature 424, 824–830 (2003). [CrossRef] [PubMed]

3.

R. W. Wood, “On a remarkable case of uneven distribution of light in a diffraction grating spectrum,” Phil. Mag. 4, 396 (1902).

4.

R. W. Wood, “Anomalous diffraction gratings,” Phys. Rev. 48, 928–936 (1935). [CrossRef]

5.

U. Fano, “The theory of anomalous diffraction gratings and of quasi-stationary waves on metallic surfaces (Sommerfeld’s waves),” J. Opt. Soc. Am. 31, 213–222 (1941). [CrossRef]

6.

S. Linden, J. Kuhl, and H. Giessen, “Controlling the interaction between light and gold nano particles: Selective suppression of extinction,” Phys. Rev. Lett. 86, 4688 (2001). [CrossRef] [PubMed]

7.

E. Kretchmann and H. Raether, “Radiative decay of nonradiative surface plasmons excited by light,” Z. Naturkorsch. A 23, 2135–2136 (1968).

8.

A. Otto, “Excitation of nonradiative surface plasma waves in silver by the method of frustrated total reflection,” Z. Phys. 216, 398 (1968). [CrossRef]

9.

J. Homola, S. S. Yee, and G. Gauglitz, “Surface plasmon resonance sensors: review,” Sensors Actuat. B 54, 3–15 (1999). [CrossRef]

10.

E. Ozbay, (Review) “Plasmonics: Merging photonics and electronics at nanoscale dimensions,” Science 311, 189–193 (2006). [CrossRef] [PubMed]

11.

S. A. Maier, P. G. Kik, H. A. Atwater, S. Meltser, E. Harel, B. E. Koel, and A. A. G. Requicha, “Local detection of electromagnetic energy transport below the diffraction limit in metal nanoparticle plasmon waveguides,” Nat. Mater. 2, 229–232 (2003). [CrossRef] [PubMed]

12.

M. I. Stockman, “Nanofocusing of optical energy in tapered plasmonic waveguides,” Phys. Rev. Lett. 93, Art. No. 137404 (2004). [CrossRef] [PubMed]

13.

J. R. Krenn and J.-C. Weeber, “Surface plasmon polaritons in metal stripes and wires,” Phil. Trans. R. Soc. Lond. A 362, 739–756 (2004). [CrossRef]

14.

D. Sarid, “Long-range surface-plasma waves on very thin metal films,” Phys, Rev. Lett. 47, 1927–1930 (1981). [CrossRef]

15.

P. Berini, “Plasmon-polariton waves guided by thin lossy metal films of finite width: Bounded modes of symmetric structures,” Phys. Rev. B 61, 10484 (2000). [CrossRef]

16.

T. Nikolajsen, K. Leosson, I. Salakhutdinov, and S. I. Bozhevolnyi, “Polymer-based surface-plasmon-polariton stripe waveguides at telecommunication wavelengths,” Appl. Phys. Lett. 82, 668–670 (2003). [CrossRef]

17.

P. Berini, R. Charbonneau, N. Lahoud, and G. Mattiussi, “Characterization of long-range surface-plasmon-polariton waveguides,” J. Appl. Phys. 98, Art. No. 043109 (2005). [CrossRef]

18.

T. Nikolajsen, K. Leosson, and S. I. Bozhevolnyi, “In-line extinction modulator based on long-range surface plasmon polaritons,” Opt. Commun. 244, 455–459 (2005). [CrossRef]

19.

S. Park and S. H. Song, “Polymeric optical attenuator based on long range surface plasmon polaritons,” Electron. Lett. 42, 402–404 (2006). [CrossRef]

20.

G. Gagnon, N. Lahoud, G. A. Mattiussi, and P. Berini, “Thermally activated variable attenuation of long-range surface plasmon-polariton waves,” J. Lightwave Technol. 24, 4391–4402 (2006). [CrossRef]

21.

A. Boltasseva, T. Nikolajsen, K. Leosson, K. Kjaer, M. S. Larsen, and S. I. Bozhevolnyi, “Integrated optical components utilizing long-range surface plasmon polaritons,” J. Lightwave technol. 23, 413–422 (2005). [CrossRef]

22.

H. S. Won, K. C. Kim, S. H. Song, C.-H. Oh, P. S. Kim, S. Park, and S. I. Kim, “Vertical coupling of long-range surface plasmon polaritons,” Appl. Phys. Lett. 88, Art. No. 011110 (2006). [CrossRef]

23.

R. Charbonneau, C. Scales, I. Breukelaar, S. Fafard, N. Lahoud, G. Mattiussi, and P. Berini, “Passive integrated optics elements based on long-range surface plasmon polaritons,” J. Lightwave Technol. 24, 477–494 (2006). [CrossRef]

24.

A. Boltasseva, S. I. Bozhevolnyi, T. Søndergaard, T. Nikolajsen, and K. Leosson, “Compact Z-add-drop wavelength filters for long-range surface plasmon polaritons,” Opt. Express 13, 4237–4243 (2005). [CrossRef] [PubMed]

25.

S. J. Charbonneau, R. Charbonneau, N. Lahoud, G. A. Mattuissi, and P. Berini, “Bragg gratings based on long-range surface plasmon-polariton waveguides: Comparison of theory and experiment,” IEEE J. Quantum Electron. 41, 1480–1491 (2005). [CrossRef]

26.

G. I. Stegeman and J. J. Burke, “Long-range surface-plasmons in electrode structures,” Appl. Phys. Lett. 43, 221–223 (1983). [CrossRef]

27.

E. N. Economou, “Surface plasmons in thin films,” Phys. Rev. 182, 539–554 (1969). [CrossRef]

28.

E. D. Palik, Handbook of Optical Constants of Solids II , (Academic Press, San Diego, 1998).

29.

M. I. Stockman, “Nanofocusing of optical energy in tapered plasmonic waveguides,” Phys. Rev. Lett. 93, Art. No. 137404 (2004). [CrossRef] [PubMed]

30.

U. Schröter and A. Dereux, “Surface plasmon polaritons on metal cylinders with dielectric core,” Phys. Rev. B 64, Art. No. 125420 (2001). [CrossRef]

OCIS Codes
(130.2790) Integrated optics : Guided waves
(250.5403) Optoelectronics : Plasmonics

ToC Category:
Optics at Surfaces

History
Original Manuscript: October 29, 2007
Revised Manuscript: November 29, 2007
Manuscript Accepted: November 29, 2007
Published: December 7, 2007

Citation
Jaewoong Yoon, Seok Ho Song, and Suntak Park, "Flat-top surface plasmon-polariton modes guided by double-electrode structures," Opt. Express 15, 17151-17162 (2007)
http://www.opticsinfobase.org/oe/abstract.cfm?URI=oe-15-25-17151


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References

  1. H. Raether, Surface plasmons on Smooth and Rough Surfaces and on Gratings, (Springer-Verlag, Berlin, 1988).
  2. W. L. Barnes, A. Dereux, and T. W. Ebbesen, (Insight review articles) "Surface plasmon subwavelength optics," Nature 424, 824-830 (2003). [CrossRef] [PubMed]
  3. R. W. Wood, "On a remarkable case of uneven distribution of light in a diffraction grating spectrum," Phil. Mag. 4, 396 (1902).
  4. R. W. Wood, "Anomalous diffraction gratings," Phys. Rev. 48, 928-936 (1935). [CrossRef]
  5. U. Fano, "The theory of anomalous diffraction gratings and of quasi-stationary waves on metallic surfaces (Sommerfeld’s waves)," J. Opt. Soc. Am. 31, 213-222 (1941). [CrossRef]
  6. S. Linden, J. Kuhl, and H. Giessen, "Controlling the interaction between light and gold nano particles: Selective suppression of extinction," Phys. Rev. Lett. 86, 4688 (2001). [CrossRef] [PubMed]
  7. E. Kretchmann and H. Raether, "Radiative decay of nonradiative surface plasmons excited by light," Z. Naturkorsch. A 23, 2135-2136 (1968).
  8. A. Otto, "Excitation of nonradiative surface plasma waves in silver by the method of frustrated total reflection," Z. Phys. 216, 398 (1968). [CrossRef]
  9. J. Homola, S. S. Yee, and G. Gauglitz, "Surface plasmon resonance sensors: review," Sensors Actuat. B 54, 3-15 (1999). [CrossRef]
  10. E. Ozbay, (Review) "Plasmonics: Merging photonics and electronics at nanoscale dimensions," Science 311, 189-193 (2006). [CrossRef] [PubMed]
  11. S. A. Maier, P. G. Kik, H. A. Atwater, S. Meltser, E. Harel, B. E. Koel, and A. A. G. Requicha, "Local detection of electromagnetic energy transport below the diffraction limit in metal nanoparticle plasmon waveguides," Nat. Mater. 2, 229-232 (2003). [CrossRef] [PubMed]
  12. M. I. Stockman, "Nanofocusing of optical energy in tapered plasmonic waveguides," Phys. Rev. Lett. 93, Art. No. 137404 (2004). [CrossRef] [PubMed]
  13. J. R. Krenn and J.-C. Weeber, "Surface plasmon polaritons in metal stripes and wires," Phil. Trans. R. Soc. Lond. A 362, 739-756 (2004). [CrossRef]
  14. D. Sarid, "Long-range surface-plasma waves on very thin metal films," Phys, Rev. Lett. 47, 1927-1930 (1981). [CrossRef]
  15. P. Berini, "Plasmon-polariton waves guided by thin lossy metal films of finite width: Bounded modes of symmetric structures," Phys. Rev. B 61, 10484 (2000). [CrossRef]
  16. T. Nikolajsen, K. Leosson, I. Salakhutdinov, and S. I. Bozhevolnyi, "Polymer-based surface-plasmonpolariton stripe waveguides at telecommunication wavelengths," Appl. Phys. Lett. 82, 668-670 (2003). [CrossRef]
  17. P. Berini, R. Charbonneau, N. Lahoud, and G. Mattiussi, "Characterization of long-range surface-plasmonpolariton waveguides," J. Appl. Phys. 98, Art. No. 043109 (2005). [CrossRef]
  18. T. Nikolajsen, K. Leosson, S. I. Bozhevolnyi, "In-line extinction modulator based on long-range surface plasmon polaritons," Opt. Commun. 244, 455-459 (2005). [CrossRef]
  19. S. Park and S. H. Song, "Polymeric optical attenuator based on long range surface plasmon polaritons," Electron. Lett. 42, 402-404 (2006). [CrossRef]
  20. G. Gagnon, N. Lahoud, G. A. Mattiussi, and P. Berini, "Thermally activated variable attenuation of longrange surface plasmon-polariton waves," J. Lightwave Technol. 24, 4391-4402 (2006). [CrossRef]
  21. A. Boltasseva, T. Nikolajsen, K. Leosson, K. Kjaer, M. S. Larsen, and S. I. Bozhevolnyi, "Integrated optical components utilizing long-range surface plasmon polaritons," J. Lightwave technol. 23, 413-422 (2005). [CrossRef]
  22. H. S. Won, K. C. Kim, S. H. Song, C.-H. Oh, P. S. Kim, S. Park, and S. I. Kim, "Vertical coupling of longrange surface plasmon polaritons," Appl. Phys. Lett. 88, Art. No. 011110 (2006). [CrossRef]
  23. R. Charbonneau, C. Scales, I. Breukelaar, S. Fafard, N. Lahoud, G. Mattiussi, and P. Berini, "Passive integrated optics elements based on long-range surface plasmon polaritons," J. Lightwave Technol. 24, 477- 494 (2006). [CrossRef]
  24. A. Boltasseva, S. I. Bozhevolnyi, T. Søndergaard, T. Nikolajsen, and K. Leosson, "Compact Z-add-drop wavelength filters for long-range surface plasmon polaritons," Opt. Express 13, 4237-4243 (2005). [CrossRef] [PubMed]
  25. S. J. Charbonneau, R. Charbonneau, N. Lahoud, G. A. Mattuissi, and P. Berini, "Bragg gratings based on long-range surface plasmon-polariton waveguides: Comparison of theory and experiment," IEEE J. Quantum Electron. 41, 1480-1491 (2005). [CrossRef]
  26. G. I. Stegeman and J. J. Burke, "Long-range surface-plasmons in electrode structures," Appl. Phys. Lett. 43, 221-223 (1983). [CrossRef]
  27. E. N. Economou, "Surface plasmons in thin films," Phys. Rev. 182, 539-554 (1969). [CrossRef]
  28. E. D. Palik, Handbook of Optical Constants of Solids II, (Academic Press, San Diego, 1998).
  29. M. I. Stockman, "Nanofocusing of optical energy in tapered plasmonic waveguides," Phys. Rev. Lett. 93, Art. No. 137404 (2004). [CrossRef] [PubMed]
  30. U. Schröter and A. Dereux, "Surface plasmon polaritons on metal cylinders with dielectric core," Phys. Rev. B 64, Art. No. 125420 (2001). [CrossRef]

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