Analytic and experimental investigations on influence of harmonic generation on acousto-optical modulation

doi:10.1364/OE.20.019168

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Analytic and experimental investigations on influence of harmonic generation on acousto-optical modulation

Peter Bechtold, Oliver Hentschel, and Michael Schmidt »View Author Affiliations

Optics Express, Vol. 20, Issue 17, pp. 19168-19175 (2012)
http://dx.doi.org/10.1364/OE.20.019168

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Abstract

In application, laser power is modulated prior to harmonic generation to a large part. Consequently modulation characteristics are influenced as a result of the non-linearity of harmonic generation. Within this paper, straight-forward approaches to calculate modulation key parameters (rise time, fall time, bandwidth and contrast ratio) of an acousto-optical modulator prior to harmonic generation stage are presented. The results will be compared to experimental data for third harmonic generation (THG) of a 1064 nm fs-laser which is power-modulated by a TeO₂-AOM prior to THG. In the latter case, rise time and fall time are significantly reduced to approximately 66% after THG both in experimental and analytical study.

1. Introduction

Acousto-optical modulators (AOMs) are commonly used to modulate laser power in intra- and extra-cavity setups [1

N. Savage, “Acousto-optic devices,” Nat. Photonics 4(10), 728–729 (2010). [CrossRef]

–5

J. H. Garcia-López, V. Aboites, A. V. Kir’yanov, M. J. Damzen, and A. Minassian, “High repetition rate Q-switching of high power Nd:YVO₄ slab laser,” Opt. Commun. 218(1-3), 155–160 (2003). [CrossRef]

]. Regarding high-power solid-state lasers, AOMs are typically used to modulate the laser’s fundamental wavelength prior to extra-cavity harmonic generation (HG), though AOMs for wavelengths ranging from UV to MID-IR are available in principle [6

R. Mazelsky and D. K. Fox, “An introduction to acousto-optic materials,” Mater. Sci. Forum 61, 1–6 (1990). [CrossRef]

]. The reasons are increased separation angles of 0th and 1st diffraction order after AOM and higher damage thresholds of acousto-optical crystals. In addition to that, modulation key parameters such as rise and fall time, contrast ratio and modulation bandwidth, are influenced by the non-linearity of the HG, i.e. preferable values result. Up to now, this beneficial influence was rarely taken into account when designing a laser system including HG and fast power modulation.

2. Analytical approach

In the following, equations for AOM power modulation of the fundamental wavelength and subsequent HG to second and third order harmonics will be given. SHG and THG are used for second and third harmonic generation (crystal) respectively. In section 2.2, the fundamental wavelength will be indexed as FUN.

2.1 Power modulation via AOM at fundamental wavelength

As preconditions to the following approach, the quotient of laser beam divergence θ₀ and acoustic beam divergence θ_a has to be smaller than 0.67 (thus limiting ellipticity of the laser beam after passage of the AOM crystal to a negligible amount) and the rise time of the RF driver voltage has to be much lower than the transit time ( = time that the acoustic wave needs to travel through the beam waist diameter 2w₀) [7

D. Maydan, “Acoustooptical pulse modulators,” IEEE J. Quantum Electron. 6(1), 15–24 (1970). [CrossRef]

I. C. Chang, “Acoustooptic devices and applications” in Handbook of Optics V, M. Bass, ed. (McGraw-Hill Professional, 2010)

]. The latter precondition is fulfilled in the majority of commercially available AOMs.

When a step function is applied to the RF driver control voltage, an acoustic wave starts to transmit through the acousto-optical crystal. The front of the acoustic wave will start to travel through the optical aperture. Thus, a fraction of the laser beam, which is assumed to be of Gaussian intensity profile, is deflected due to diffraction. The amount of the diffracted laser power is dependent on the position of the front of the acoustic wave, i.e. time, and is derived as follows.

A Gaussian intensity distribution I(x,y) equals Eq. (1), where I₀ is the peak intensity at x = 0 and y = 0 (r = 0) and w₀ the 1/e² beam radius [9

J. M. Khosrofian and B. A. Garetz, “Measurement of a gaussian laser beam diameter through the direct inversion of knife-edge data,” Appl. Opt. 22(21), 3406–3410 (1983). [CrossRef] [PubMed]

I (x, y) = I_{0} \exp (- \frac{2 r^{2}}{w_{0}^{2}}) = I_{0} \exp (- \frac{2 (x^{2} + y^{2})}{w_{0}^{2}})

(1)

The deflected, i.e. modulated average power P(t) is then given by Eq. (2), cp. knife-edge method [9

J. M. Khosrofian and B. A. Garetz, “Measurement of a gaussian laser beam diameter through the direct inversion of knife-edge data,” Appl. Opt. 22(21), 3406–3410 (1983). [CrossRef] [PubMed]

], with x = Vt being the position of the front of the acoustic wave, where V equals the acoustic wave velocity, and the total laser power is P₀ = ½πI₀w₀².

P (t) = \int_{- \infty}^{x} \int_{- \infty}^{\infty} I (x, y) d y d x = \frac{1}{2} P_{0} (1 + e r f (\sqrt{2} \frac{V t}{w_{0}}))

(2)

To derive rise and fall times from Eq. (2), t is calculated for P(t)/P₀ = 0.1 and 0.9 respectively and Eq. (3) is obtained.

t_{r i s e} = t_{f a l l} = t (P (t) / P_{0} = 0.9) - t (P (t) / P_{0} = 0.1) = 1.28 \frac{w_{0}}{V}

(3)

As rise and fall times are equivalent due to symmetry, the modulation bandwidth f_m results from Eq. (4) (derived from [7

D. Maydan, “Acoustooptical pulse modulators,” IEEE J. Quantum Electron. 6(1), 15–24 (1970). [CrossRef]

]). Results for t_rise/fall and f_m are in accordance with [8

I. C. Chang, “Acoustooptic devices and applications” in Handbook of Optics V, M. Bass, ed. (McGraw-Hill Professional, 2010)

f_{m} \approx 0.5 \frac{2}{(t_{r i s e} + t_{f a l l})} = 0.78 \frac{V}{2 w_{0}}

(4)

2.2 Power modulation after harmonic generation

For harmonic generation, optimal alignment (no phase-mismatch) and collinear waves are presumed. The intensity of the second harmonic beam I_SHG(x,y) can be expressed by Eq. (5) [10

B. E. A. Saleh and M. C. Teich, Fundamentals of Photonics (Wiley Series in Pure & Applied Optics, 2007), Chap. 21.

, 11

D. Eimerl, “High average power harmonic generation,” IEEE J. Quantum Electron. 23(5), 575–592 (1987). [CrossRef]

], where L is the interaction length, d_eff the effective non-linear coefficient (with m/V as unit), ε₀ the dielectric constant (ε₀ = 8.854 10⁻¹² F/m), ω = 2π c₀/λ_FUN the angular frequency and Ζ = Ζ₀/n the impedance (Z₀ = 377 Ω). The intensity profile I_FUN(x,y) is equivalent to Eq. (1), with the difference of using I_FUN0 for the peak intensity of the fundamental laser beam (instead of I₀) and w_FUN for the 1/e² beam diameter of the fundamental laser beam when transmitting through the SHG crystal (instead of w₀). As a pulsed laser is used in the experiments, it is chosen that

I_{F U N 0}

equals

I_{F U N 0} = {(2 f_{r e p} τ)}^{- 1} \cdot (2 P_{F U N} / π w_{F U N}^{2}) = P_{F U N} / π w_{F U N}^{2} f_{r e p} τ

to rate the dependence of HG efficiency on laser peak power, where P_FUN is the average fundamental laser power, f_rep the repetition rate of the laser and τ FWHM the pulse duration (sech² shape assumed). This proved to be most adequate as approximation, though it has to be noted that other pre-factors for

I_{F U N 0}

may be chosen. Further, τ is assumed to be unaffected by HG, i.e. constant.

I_{S H G} (x, y) = I_{F U N} (x, y) \tan h^{2} (Θ_{S H G} \sqrt{I_{F U N} (x, y)})

(5)

Θ_{S H G} = L_{S H G} d_{e f f, S H G} ε_{0} ω \sqrt{2 Z_{S H G}^{3}}

(6)

Third harmonic generation (THG) is realized via sum frequency generation of the SHG laser beam as signal and the residual fundamental laser beam as pump. With this precondition, the intensity after THG can be expressed by Eq. (7) [10

B. E. A. Saleh and M. C. Teich, Fundamentals of Photonics (Wiley Series in Pure & Applied Optics, 2007), Chap. 21.

]. The residual pump intensity equals I_FUN - I_SHG due to previous SHG conversion. For low SHG conversion efficiency, the residual fundamental pump intensity can be estimated as I_FUN - I_SHG ≈I_FUN.

I_{T H G} (x, y) = \frac{3}{2} I_{S H G} (x, y) \sin^{2} (Θ_{T H G} \sqrt{I_{F U N} (x, y) - I_{S H G} (x, y)})

(7)

Θ_{T H G} = 2 L_{T H G} d_{e f f, T H G} ε_{0} ω \sqrt{3 Z_{T H G}^{3}}

(8)

Variables Θ_SHG (Eq. (6)) and Θ_THG (Eq. (8)) summarize all non-variant parameters for SHG or THG respectively (dependent on fundamental wavelength, crystal geometry and crystal material). Subsequently, the temporal shape of the modulated average power after THG can be calculated using Eq. (9), cp. Equation (2). The upper limit of integration over x equals (w_FUN/w₀)Vt, i.e. it is assumed that the intensity profile after AOM is reimaged to HG according to geometrical optics. w_FUN and w₀ are the beam radii at fundamental wavelength in the HG crystals and AOM crystal respectively.

P_{T H G} (t) = 2 f_{r e p} τ \int_{- \infty}^{\frac{w_{F U N}}{w_{0}} V t} \int_{- \infty}^{\infty} I_{T H G} (x, y) d y d x

(9)

Equation (9) is derived under the precondition that the truncated laser beam (truncated due to the working principle of AOM) will transmit to SHG and THG crystals in diffraction-free manner, which is not true in the real case. I.e. truncation will generally blur within a short range or due to additional focussing before HG. To take this fact into account, a second, simpler approach with following assumptions is eligible.

A mean intensity I_FUN is used (instead of Eq. (1)) and set as I_FUN(x,y) = I_FUN,0/2 = P_FUN/(A_FUNf_repτ) for

r^{2} = x^{2} + y^{2} = 0_{} {..}_{} 2 w_{F U N}^{2}

, otherwise I = 0. The interaction area A_FUN is therefore

A_{F U N} = 2 π w_{F U N}^{2}

. The same accounts for I_SHG(x,y) and I_THG(x,y) with according indices. Further, it is assumed that the beam radius is unaffected by HG, i.e. w_FUN = w_SHG = w_THG (further analysis proves minor impact of this simplification on resulting shapes of P_SHG(t) and P_THG(t)). As a result, Eq. (5) can be rewritten as Eqs. (10) and (11).

P_{S H G} (t) = P (t) \tan h^{2} (Θ_{S H G}^{*} \sqrt{P (t)})

(10)

Θ_{S H G}^{*} = Θ_{S H G} \sqrt{\frac{1}{2 π w_{F U N}^{2} f_{r e p} τ}}

(11)

The same accounts for Eqs. (7), (12), and (13) result. As a remark, Eq. (12) expresses the temporal shape of the modulated laser power analytically, where Eq. (9) has to be solved numerically generally.

P_{T H G} (t) = \frac{3}{2} P_{S H G} (t) \sin^{2} (Θ_{T H G}^{*} \sqrt{P (t) - P_{S H G} (t)})

(12)

Θ_{T H G}^{*} = Θ_{T H G}^{} \sqrt{\frac{1}{2 π w_{F U N}^{2} f_{r e p} τ}}

(13)

As before, Θ*_SHG and Θ*_THG summarize all non-variant variables, now including fundamental laser beam characteristics. Calculated values for Θ_SHG, Θ*_SHG, Θ_THG and Θ*_THG are expected to be higher than experimentally derived values due to neglection of walkoff, dephasing, group velocity delay and other effects. It has to be noted that there are more detailed ways to calculate SHG and THG conversion efficiencies such as [11

D. Eimerl, “High average power harmonic generation,” IEEE J. Quantum Electron. 23(5), 575–592 (1987). [CrossRef]

, 12

J. A. Armstrong, N. N. Bloembergen, J. Ducuing, and P. S. Pershan, “Interactions between light waves in a nonlinear dielectric,” Phys. Rev. 127(6), 1918–1939 (1962). [CrossRef]

]. However, for anticipated usage, the formulas stated proved to be more than adequate.

Resulting t_{rise/fall,SHG} after SHG can be calculated using Eqs. (6) or (10) as t_rise,SHG = t_fall,SHG = t(P_SHG/P_0,SHG = 0.9) – t(P_SHG/P_0,SHG = 0.1), where P_0,SHG is the maximum power after SHG. As long as the shape of P_SHG(t)/P_0,SHG does not significantly differ from P(t)/P₀, the bandwidth f_m,SHG can still be estimated to f_m,SHG ≅ 0.502 2/(t_rise,SHG + t_fall,SHG). Both predications apply to t_{rise/fall,THG} and f_m,THG the same way when using Eqs. (9) or (12).

3. Experimental setup

The experimental setup consists of a fs-laser, an AOM modulating the laser power at fundamental wavelength, and a THG module. The laser power is measured with a Coherent LM-3 thermopile power meter for powers >30 mW and a Coherent LM2-UV silicon diode power meter for powers <30 mW. Rise time, fall time and contrast ratio are measured using a Tektronix TDS-3034C 300 MHz oscilloscope with a Thorlabs FDS010 silicon photodiode (1 ns rise time) as detector. As one oscilloscope trace of fs-pulses is not sufficient for analysis (1 µs pulse pause between two fs pulses), repetitive oscilloscope traces are collected and overlaid over each other via a long time of oscilloscope screen persistence (~10 s).

The fs-laser is emitting pulses at a repetition rate f_rep = 1 MHz with a FWHM pulse duration τ = 400 fs (assuming sech² pulse shape), wavelength λ = 1064 nm and max. pulse energy E_p,max = 2.0 µJ. The RMS pulse-to-pulse stability is approximately 1% and M² ≅ 1.25. The laser beam is collimated to w₀ = 0.49 mm via a Galilei-type telescope prior to the AOM.

Modulation is realized by an AOM (AA optoelectronic MT80-A1.5-1064) with TeO₂ as crystal material (V = 4200 m/s). The AOM system aperture equals 1.5 x 2 mm², thus only slight clipping of the laser beam will occur. At 80 MHz carrier frequency of the acoustic wave and RF power of 2.0 W, the AOM is specified to a contrast ratio >2000:1, rise time 160 ns at 1 mm 1/e² beam diameter and diffraction efficiency of >85%. The separation angle of 0th and 1st order beams is 20 mrad.

The diffracted (thus modulated) 1st order laser beam is focused into the middle of the frequency doubling crystal of 5 mm thickness via a second Galilei-type telescope. The resulting focal spot radius equals approximately 250 µm (Rayleigh length ~152 mm). LiB₂O₅ (LBO) is used as SHG crystal material. Polarization and crystal angle are aligned for optimal critical phase matching and SH conversion efficiency of Type I SHG (d_eff,SHG ≅ 0.82 10⁻¹² m/V [13

S. P. Velsko, M. Webb, L. Davis, and C. Huang, “Phase-matches harmonic generation in lithium triborate (LBO),” IEEE J. Quantum Electron. 27(9), 2182–2192 (1991). [CrossRef]

]).

After SHG the polarization of the residual fundamental beam is rotated by π/2 for subsequent Type I THG via a crystal quartz waveplate (phase retardation λ/2 for 1064 nm and λ for 532 nm). LBO of 3 mm thickness is used as THG crystal. No delay compensation between fundamental and SH beam is used. Thus, THG efficiency will be sub-optimal to some extent. As before, the crystal angle is aligned for optimal phase matching and TH conversion efficiency (d_eff,THG ≅ 0.67 pm/V [13

S. P. Velsko, M. Webb, L. Davis, and C. Huang, “Phase-matches harmonic generation in lithium triborate (LBO),” IEEE J. Quantum Electron. 27(9), 2182–2192 (1991). [CrossRef]

]). No additional focussing takes place before THG (due to Rayleigh length >> separation between SHG and THG crystals). After THG, residual light of SH and fundamental wavelength is subtracted by a dichroitic mirror.

The experimental setup is depicted in Fig. 1 schematically.

Fig. 1 Schematical layout of experimental setup.

The resulting average THG laser power in dependence to average fundamental laser power is depicted in Fig. 2 . Equations (9) and (12) for t→∞ are fitted to the experimentally obtained values, where Θ_SHG and Θ_THG or Θ*_SHG and Θ*_THG respectively are used as independent variables.

Fig. 2 Average THG power vs. average fundamental power. Polynomial regression equals Eq. (14). Regression of Eq. (9) is for Θ_SHG = 2.88 10⁻⁷ W^-1/2m and Θ_THG = 1.02 10⁻⁷ W^-1/2m. Regression of Eq. (12) is for Θ*_SHG = 0.843 W^-1/2 and Θ*_THG = 0.251 W^-1/2. Max. value of experimental P_THG/P_FUN equals 3.4% at P_FUN = 1.51 W. Plots of regressions of Eq. (9) and Eq. (12) are exactly on each other.

Additionally, a polynomial fit of fourth order (P_THG(P) = a P⁴ + b P³ + c P² + d P + e) is shown in Fig. 2 for comparison. In the latter case, the independent variables d and e are set to zero, to represent P_THG(0) = 0 and dP_THG(0)/dP_FUN = 0. Polynomial fits of lower order (2nd, 3rd) delivered less accurate agreement between regression and experimental values. Polynomial fits of higher order (5th, 6th) did not increase agreement significantly. This is understandable when solving Eqs. (10) and (12) for low values of P(t). P_THG then becomes P_THG ~P(t)³ - Θ*_SHG² P(t)⁴. The polynomial fit equals Eq. (14).

P_{T H G} = - 0.00714 P^{4} + 0.0164 P^{3} + 0.0138 P^{2}

(14)

Θ_SHG, Θ_THG, Θ*_SHG and Θ*_THG are calculated using the stated parameters and Eqs. (6), (8), (11), and (13). Due to missing delay compensation, the experimentally obtained values for Θ_THG and Θ*_THG are significantly lower than the calculated values as of neglection of group velocity delay. Results of calculated and experimentally derived values are summarized in Table 1 .

Table 1 Results forΘ_SHG, Θ_THG, Θ*_SHG and Θ*_THG

	Θ_SHG	Θ*_SHG	Θ_THG	Θ*_THG
	10⁻⁷ W^-1/2m	W^-1/2	10⁻⁷ W^-1/2m	W^-1/2
Calculated via Eqs. (6), (8), (11), (13)	3.41	0.862	4.10	1.04
Regression of Eq. (9)	2.88	-	1.02	-
Regression of Eq. (12)	-	0.843	-	0.251

3. Experimental results

In the following, experimental results on modulation key parameters both prior to and after THG are presented. Analytical results for Eqs. (9), (12) and (14) will be compared, where the values for Θ_SHG, Θ_THG, Θ*_SHG and Θ*_THG correspond to the values of regressions in Table 1. In all diagrams, experimental results are shown as point plots and calculated results as line plots.

3.1 Temporal AOM modulation shape prior to and after THG

The temporal development of modulated laser power is measured. Analytical results for the temporal development before THG are derived according to Eq. (3). Experimental and analytical results are depicted in Fig. 3 for both max. average fundamental power before THG P_FUN = 1.51 W (Fig. 3 left) and P_FUN = 0.36 W (Fig. 3 right).

Fig. 3 Temporal development of normalized average power prior to and after THG.

3.2 Dependence of modulation parameters on THG efficiency

Rise and fall times are measured. Before THG, the rise time equals 156 ns and the fall time 148 ns (independent on P_FUN). The average value of 152 ns is in good accordance with the specification of 160 ns/mm ⋅ 0.98 mm = 157 ns. Rise and fall times after THG are measured for varying average fundamental power P_FUN, thus varying THG efficiency. Analytical results are provided by solving both P_THG(t_90%) = 0.9P_THG,max and P_THG(t_10%) = 0.1P_THG,max for t_rise/fall = t_90% - t_10% with numerical methods. The bandwidth f_m is calculated via Eq. (4) and equals 3.3 MHz before THG. The results are depicted in Fig. 4 , where the upper limit of the rise/fall time ordinate and lower limit of the bandwidth ordinate are set to the value prior to THG.

Fig. 4 Rise/fall time t_rise/fall and bandwidth f_m vs. average THG power P_THG. Upper limit of t_rise/fall and lower limit of f_m equal values before THG (152 ns and 3.3 MHz respectively).

The contrast ratio before THG is measured and equals 3125:1, which exceeds the specification of 2000:1. At max. average power of the fundamental laser beam P_FUN = 1.51 W, analytical values of the contrast ratio after THG exceed 10⁹:1 for Eq. (9) and (12) and 10⁷:1 for Eq. (14). Experimentally, the contrast ratio after THG is higher than the signal-to-noise-ratio of the diode signal of 10⁴:1.

4. Discussion

Experimentally, a significant reduction of rise and fall time of the AOM after THG down to 60% … 71% of rise and fall time prior to THG is proved for THG efficiencies P_FUN/P_THG > 1% (P_THG > 5 mW), cp. Figure 4. This results in a raise of bandwidth to 141% … 152% compared to the value prior to THG. For low THG efficiencies of < 1% (P_THG < 5 mW), rise and fall times slightly increase apparently. Neither model represents this. The effect is accredited to leakage of the SHG and fundamental laser beam after the dichroitic mirror. Sensitivity of the photodiode used in experiments is 7 times higher for 532 nm compared to 355 nm and 1064 nm. Solving Eq. (10), the rise time at 532 nm is approximately 125 ns. The rise time at the fundamental wavelength is 152 ns. A leakage of the SHG laser beam of ~0.2 mW, fundamental laser beam of ~1 mW or a combination of both therefore explains the deviation.

The analytical solution via Eq. (9) – the integration of the THG intensity profile under assumption of diffraction-free propagation of laser beams – does not represent the measured time delay between temporal modulated average power development prior to and after THG, which is measured to be in a range of 20 ns .. 40 ns, cp. Figure 2. This can directly be appointed to neglection of diffraction. Then again, Eq. (9) delivers values for rise and fall times which deviate from the experimental ones less than +/− 8% for THG efficiencies > 1.5% (P_THG > 10 mW).

The simplified model via Eq. (12), which delivers an analytical solution for temporal modulated power development, neglects truncation of the beam and therefore represents time delay well, cp. Figure 2. The values for rise and fall time are stable over a wide interval and deviate from the experimental ones by + 5% … + 15% for THG efficiencies > 1% (P_THG > 5 mW).

The direct polynomial solution, Eq. (14), shows similar behavior as Eq. (12), but it has to be noted that it does not represent the physical properties of the HG process and therefore will not be useful to estimate values far away from the regression interval (e.g. THG efficiency > 3.5%).

The contrast ratio after THG is exceeding the measurement range towards excellent values of >10⁴:1.

5. Summary and outlook

The experimental results show a significant reduction of rise and fall time of laser power modulated via AOM due to harmonic generation. The quotient of rise and fall time prior to THG (directly after AOM) to after THG equals ~0.66, thus the bandwidth is increased by a factor of ~1.5. This quotient is directly correlated to the characteristics of harmonic generation, i.e. its non-linearity. Also due to non-linearity, the temporal development of the modulated laser power is delayed by approximately 30 ns.

Two analytical methods to estimate modulation parameters after THG are introduced. On the one hand Eq. (9) is well suited to calculate resulting rise and fall times to an accuracy of +/− 8% but does not represent the temporal delay of the modulation. On the other hand Eq. (12) represents the delay very well, and results for rise and fall time after HG deviate from the experimental values by + 5% … + 15%. Therefore both methods are suited to predict the behavior after HG, where Eq. (12) is simpler to use, since no numerical methods have to be applied to gain the temporal development of the modulated power after HG.

With small adaptions, the presented methods are applicable to other harmonic generations, such as FHG or direct THG (not via sum frequency, but direct tripling of the fundamental wavelength). The same accounts to other modulation devices, such as electro-optic (e.g. pockels cell) or interferometric modulators (e.g. Mach-Zehnder modulator). Mainly Eq. (1) and Eq. (2) would have to be changed in the latter case.

Acknowledgments

The authors would like to thank Wavelight GmbH (part of Alcon Inc.) for continuous cooperation throughout the project and Medical Valley EMN e.V. for general support. Furthermore the authors gratefully acknowledge the financial support by and scientific exchange with the Erlangen Graduate School in Advanced Optical Technologies (SAOT) by the German Research Foundation (DFG), the framework of the German excellence initiative. This project is supported by the German Federal Ministry of Education and Research (BMBF), project grant No. 01EX1011C.

References and links

1.	N. Savage, “Acousto-optic devices,” Nat. Photonics 4(10), 728–729 (2010). [CrossRef]
2.	A. W. Warner and D. A. Pinnow, “Miniature acousto-optic modulators for optical communications,” IEEE J. Quantum Electron. 9(12), 1155–1157 (1973). [CrossRef]
3.	A. J. DeMaria, R. Gagosz, and G. Barnard, “Ultrasonic-refraction shutter for optical master oscillators,” Appl. Phys. (Berl.) 34, 453–456 (1963).
4.	D. Maydan, “Fast modulator for extraction of internal laser power,” Appl. Phys. (Berl.) 41, 1552–1559 (1970).
5.	J. H. Garcia-López, V. Aboites, A. V. Kir’yanov, M. J. Damzen, and A. Minassian, “High repetition rate Q-switching of high power Nd:YVO₄ slab laser,” Opt. Commun. 218(1-3), 155–160 (2003). [CrossRef]
6.	R. Mazelsky and D. K. Fox, “An introduction to acousto-optic materials,” Mater. Sci. Forum 61, 1–6 (1990). [CrossRef]
7.	D. Maydan, “Acoustooptical pulse modulators,” IEEE J. Quantum Electron. 6(1), 15–24 (1970). [CrossRef]
8.	I. C. Chang, “Acoustooptic devices and applications” in Handbook of Optics V, M. Bass, ed. (McGraw-Hill Professional, 2010)
9.	J. M. Khosrofian and B. A. Garetz, “Measurement of a gaussian laser beam diameter through the direct inversion of knife-edge data,” Appl. Opt. 22(21), 3406–3410 (1983). [CrossRef] [PubMed]
10.	B. E. A. Saleh and M. C. Teich, Fundamentals of Photonics (Wiley Series in Pure & Applied Optics, 2007), Chap. 21.
11.	D. Eimerl, “High average power harmonic generation,” IEEE J. Quantum Electron. 23(5), 575–592 (1987). [CrossRef]
12.	J. A. Armstrong, N. N. Bloembergen, J. Ducuing, and P. S. Pershan, “Interactions between light waves in a nonlinear dielectric,” Phys. Rev. 127(6), 1918–1939 (1962). [CrossRef]
13.	S. P. Velsko, M. Webb, L. Davis, and C. Huang, “Phase-matches harmonic generation in lithium triborate (LBO),” IEEE J. Quantum Electron. 27(9), 2182–2192 (1991). [CrossRef]

OCIS Codes
(140.7090) Lasers and laser optics : Ultrafast lasers
(190.2620) Nonlinear optics : Harmonic generation and mixing
(220.4830) Optical design and fabrication : Systems design
(230.1040) Optical devices : Acousto-optical devices
(230.4110) Optical devices : Modulators

ToC Category:
Lasers and Laser Optics

History
Original Manuscript: May 23, 2012
Manuscript Accepted: July 19, 2012
Published: August 6, 2012

Citation
Peter Bechtold, Oliver Hentschel, and Michael Schmidt, "Analytic and experimental investigations on influence of harmonic generation on acousto-optical modulation," Opt. Express 20, 19168-19175 (2012)
http://www.opticsinfobase.org/oe/abstract.cfm?URI=oe-20-17-19168

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References

N. Savage, “Acousto-optic devices,” Nat. Photonics4(10), 728–729 (2010). [CrossRef]
A. W. Warner and D. A. Pinnow, “Miniature acousto-optic modulators for optical communications,” IEEE J. Quantum Electron.9(12), 1155–1157 (1973). [CrossRef]
A. J. DeMaria, R. Gagosz, and G. Barnard, “Ultrasonic-refraction shutter for optical master oscillators,” Appl. Phys. (Berl.)34, 453–456 (1963).
D. Maydan, “Fast modulator for extraction of internal laser power,” Appl. Phys. (Berl.)41, 1552–1559 (1970).
J. H. Garcia-López, V. Aboites, A. V. Kir’yanov, M. J. Damzen, and A. Minassian, “High repetition rate Q-switching of high power Nd:YVO4 slab laser,” Opt. Commun.218(1-3), 155–160 (2003). [CrossRef]
R. Mazelsky and D. K. Fox, “An introduction to acousto-optic materials,” Mater. Sci. Forum61, 1–6 (1990). [CrossRef]
D. Maydan, “Acoustooptical pulse modulators,” IEEE J. Quantum Electron.6(1), 15–24 (1970). [CrossRef]
I. C. Chang, “Acoustooptic devices and applications” in Handbook of Optics V, M. Bass, ed. (McGraw-Hill Professional, 2010)
J. M. Khosrofian and B. A. Garetz, “Measurement of a gaussian laser beam diameter through the direct inversion of knife-edge data,” Appl. Opt.22(21), 3406–3410 (1983). [CrossRef] [PubMed]
B. E. A. Saleh and M. C. Teich, Fundamentals of Photonics (Wiley Series in Pure & Applied Optics, 2007), Chap. 21.
D. Eimerl, “High average power harmonic generation,” IEEE J. Quantum Electron.23(5), 575–592 (1987). [CrossRef]
J. A. Armstrong, N. N. Bloembergen, J. Ducuing, and P. S. Pershan, “Interactions between light waves in a nonlinear dielectric,” Phys. Rev.127(6), 1918–1939 (1962). [CrossRef]
S. P. Velsko, M. Webb, L. Davis, and C. Huang, “Phase-matches harmonic generation in lithium triborate (LBO),” IEEE J. Quantum Electron.27(9), 2182–2192 (1991). [CrossRef]

Aboites, V.
Armstrong, J. A.
Barnard, G.
Bloembergen, N. N.
Damzen, M. J.
Davis, L.
DeMaria, A. J.
Ducuing, J.
Eimerl, D.
Fox, D. K.
Gagosz, R.
Garcia-López, J. H.
Garetz, B. A.
Huang, C.
Khosrofian, J. M.
Kir’yanov, A. V.
Maydan, D.
Mazelsky, R.
Minassian, A.
Pershan, P. S.
Pinnow, D. A.
Savage, N.
Velsko, S. P.
Warner, A. W.
Webb, M.

Appl. Opt.

J. M. Khosrofian and B. A. Garetz, “Measurement of a gaussian laser beam diameter through the direct inversion of knife-edge data,” Appl. Opt.22(21), 3406–3410 (1983). [CrossRef] [PubMed]

Appl. Phys. (Berl.)

A. J. DeMaria, R. Gagosz, and G. Barnard, “Ultrasonic-refraction shutter for optical master oscillators,” Appl. Phys. (Berl.)34, 453–456 (1963).
D. Maydan, “Fast modulator for extraction of internal laser power,” Appl. Phys. (Berl.)41, 1552–1559 (1970).

IEEE J. Quantum Electron.

A. W. Warner and D. A. Pinnow, “Miniature acousto-optic modulators for optical communications,” IEEE J. Quantum Electron.9(12), 1155–1157 (1973). [CrossRef]
D. Maydan, “Acoustooptical pulse modulators,” IEEE J. Quantum Electron.6(1), 15–24 (1970). [CrossRef]
D. Eimerl, “High average power harmonic generation,” IEEE J. Quantum Electron.23(5), 575–592 (1987). [CrossRef]
S. P. Velsko, M. Webb, L. Davis, and C. Huang, “Phase-matches harmonic generation in lithium triborate (LBO),” IEEE J. Quantum Electron.27(9), 2182–2192 (1991). [CrossRef]

Mater. Sci. Forum

R. Mazelsky and D. K. Fox, “An introduction to acousto-optic materials,” Mater. Sci. Forum61, 1–6 (1990). [CrossRef]

Nat. Photonics

N. Savage, “Acousto-optic devices,” Nat. Photonics4(10), 728–729 (2010). [CrossRef]

Opt. Commun.

J. H. Garcia-López, V. Aboites, A. V. Kir’yanov, M. J. Damzen, and A. Minassian, “High repetition rate Q-switching of high power Nd:YVO4 slab laser,” Opt. Commun.218(1-3), 155–160 (2003). [CrossRef]

Phys. Rev.

J. A. Armstrong, N. N. Bloembergen, J. Ducuing, and P. S. Pershan, “Interactions between light waves in a nonlinear dielectric,” Phys. Rev.127(6), 1918–1939 (1962). [CrossRef]

Other

I. C. Chang, “Acoustooptic devices and applications” in Handbook of Optics V, M. Bass, ed. (McGraw-Hill Professional, 2010)
B. E. A. Saleh and M. C. Teich, Fundamentals of Photonics (Wiley Series in Pure & Applied Optics, 2007), Chap. 21.

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