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Jang, H., Viotti, A-L., Strömqvist, G., Zukauskas, A., Canalias, C. et al. (2017)Counter-propagating parametric interaction with phonon-polaritons in periodically poledKTiOPO4.Optics Express, 25(3): 2677-2686https://doi.org/10.1364/OE.25.002677

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Counter-propagating parametric interaction with phonon-polaritons in periodically poled KTiOPO4

HOON JANG, ANNE-LISE VIOTTI, GUSTAV STRÖMQVIST, ANDRIUS ZUKAUSKAS, CARLOTA CANALIAS, AND VALDAS PASISKEVICIUS

* Department of Applied Physics, KTH - Royal Institute of Technology, Roslagstullsbacken 21, 10691, Stockholm, Sweden *[email protected]

Abstract: Strongly enhanced backward stimulated polariton scattering (BSPS) is demonstrated in periodically-poled KTiOPO4 (KTP) crystals with a high power-conversion efficiency up to 70%. We study the physical mechanism of such counter-propagating parametric interaction with phonon-polaritons in χ(2) modulated structures. BSPS is a three-wave mixing that is distinguished from backward stimulated Raman scattering (BSRS), while a strong absorption at large polariton wave-vectors can still make BSPS display certain characteristics of BSRS such as self-compression of the Stokes pulse. We also compare BSPS with counter-propagating parametric oscillation in the near- and mid-infrared range, providing an estimation of the fabrication error margin to expect the outcome of their competition in the same device. © 2017 Optical Society of America

OCIS codes: (290.5910) Scattering, stimulated Raman; (190.4400) Nonlinear optics, materials; (130.2260) Ferroelectrics; (130.3060) Infrared; (300.6495) Spectroscopy, terahertz.

References and links

1. U. Schwarz and M. Maier, “Damping mechanisms of phonon polaritons, exploited by stimulated Raman gain measurements,” Phys. Rev. B 58(2), 766–775 (1998).

2. B. Bittner, M. Scherm, T. Schoedl, T. Tyroller, U. T. Schwarz, and M. Maier, “Phonon-polariton damping by low-frequency excitations in lithium tantalate investigated by spontaneous and stimulated Raman scattering,” J. Phys. Condens. Matter 14(39), 9013–9028 (2002).

3. H. J. Bakker, S. Hunsche, and H. Kurz, “Investigation of anharmonic lattice vibrations with coherent phonon polaritons,” Phys. Rev. B Condens. Matter 50(2), 914–920 (1994).

4. V. Pasiskevicius, C. Canalias, and F. Laurell, “Highly efficient stimulated Raman scattering of picosecond pulses in KTiOPO4,” Appl. Phys. Lett. 88(4), 041110 (2006).

5. A. A. Maradudin and S. Ushioda, “A theory of the first order Raman scattering of light by polaritons in crystals of the rocksalt structure,” J. Phys. Chem. Solids 31(5), 1075–1083 (1970).

6. D. Heiman, “Magneto-optic Raman scattering of Raman-inactive phonon polaritons,” J. Appl. Phys. 51(6), 3354–3358 (1980).

7. C. Flytzanis, “Electro-optic coefficients in III-V compounds,” Phys. Rev. Lett. 23(23), 1336–1339 (1969). 8. C. H. Hanry and C. G. B. Garret, “Theory of parametric gain near a lattice resonance,” Phys. Rev. 171(3), 1058–

1064 (1968). 9. W. L. Faust, C. H. Henry, and R. H. Eick, “Dispersion inthe nonlinear susceptibility of GaP near the restrahl

band,” Phys. Rev. 173(3), 781–786 (1968). 10. A. Mayer and F. Keilmann, “Far-infrared nonlinear optics. I. χ (2) near ionic resonance,” Phys. Rev. B Condens.

Matter 33(10), 6954–6961 (1986). 11. E. Yablonovitch, C. Flytzanis, and N. Bloembergen, “Anisotropic interference of three-wave and double two-

wave frequency mixing in GaAs,” Phys. Rev. Lett. 29(13), 865–868 (1972). 12. H. Jang, G. Strömqvist, V. Pasiskevicius, and C. Canalias, “Control of forward stimulated polariton scattering in

periodically-poled KTP crystals,” Opt. Express 21(22), 27277–27283 (2013). 13. K. Suizu and K. Kawase, “Monochromatic-tunable Terahertz-wave sources based on nonlinear frequency

conversion using Lithium Niobate crystal,” IEEE J. Sel. Top. Quantum Electron. 14(2), 295–306 (2008). 14. W. Wang, Z. Cong, X. Chen, X. Zhang, Z. Qin, G. Tang, N. Li, C. Wang, and Q. Lu, “Terahertz parametric

oscillator based on KTiOPO4 crystal,” Opt. Lett. 39(13), 3706–3709 (2014). 15. W. Wang, Z. Cong, Z. Liu, X. Zhang, Z. Qin, G. Tang, N. Li, Y. Zhang, and Q. Lu, “THz-wave generation via

stimulated polariton scattering in KTiOAsO4 crystal,” Opt. Express 22(14), 17092–17098 (2014).

Vol. 25, No. 3 | 6 Feb 2017 | OPTICS EXPRESS 2677

#282198 https://doi.org/10.1364/OE.25.002677 Journal © 2017 Received 5 Dec 2016; revised 24 Jan 2017; accepted 25 Jan 2017; published 1 Feb 2017

16. N. Ocelic and R. Hillenbrand, “Subwavelength-scale tailoring of surface phonon polaritons by focused ion-beam implantation,” Nat. Mater. 3(9), 606–609 (2004).

17. N. S. Stoyanov, D. W. Ward, T. Feurer, and K. A. Nelson, “Terahertz polariton propagation in patterned materials,” Nat. Mater. 1(2), 95–98 (2002).

18. P. Peier, H. Merbold, V. Pahinin, K. A. Nelson, and T. Feurer, “Imaging of THz waves in 2D photonic crystal structures embedded in a slab waveguide,” New J. Phys. 12(1), 013014 (2010).

19. J. A. L’Huillier, G. Torosyan, M. Theuer, C. Rau, Y. Avetisyan, and R. Beigang, “Generation of THz radiation using bulk, periodically and aperiodically poled lithium niobate – Part 2: Experiments,” Appl. Phys. B 86(2), 197–208 (2007).

20. Y.-S. Lee, T. Meade, V. Perlin, H. Winful, T. B. Norris, and A. Galvanauskas, “Generation of narrow-band terahertz radiation via optical rectification of femtosecond pulses in periodically poled lithium niobate,” Appl. Phys. Lett. 76(18), 2505–2507 (2000).

21. N. E. Yu, M. Oh, H. Kang, C. Jung, B. H. Kim, K. Lee, D. Ko, S. Takekawa, and K. Kitamura, “Continuous tuning of a narrow-band terahertz wave in periodically poled stoichiometric LiTaO3 crystal with a fan-out grating structure,” Appl. Phys. Express 7(1), 012101 (2014).

22. T. Buma and T. B. Norris, “Coded excitation of broadband terahertz using optical rectification in poled lithium niobate,” Appl. Phys. Lett. 87(25), 251105 (2005).

23. M. P. Hasselbeck, L. A. Schlie, and D. Stalnaker, “Emission of electromagnetic radiation by coherent vibrational waves in stimulated Raman scattering,” Appl. Phys. Lett. 85(2), 173–175 (2004).

24. M. Sotome, N. Kida, R. Takeda, and H. Okamoto, “Terahertz radiation induced by coherent phonon generation via impulsive stimulated Raman scattering in paratellurite,” Phys. Rev. A 90(3), 033842 (2014).

25. D. Molter, M. Theuer, and R. Beigang, “Nanosecond terahertz optical parametric oscillator with a novel quasi phase matching scheme in lithium niobate,” Opt. Express 17(8), 6623–6628 (2009).

26. D. A. Walsh, P. G. Browne, M. H. Dunn, and C. F. Rae, “Intracavity parametric generation of nanosecond terahertz radiation using quasi-phase-matching,” Opt. Express 18(13), 13951–13963 (2010).

27. M. Maier, W. Kaiser, and J. A. Giordmaine, “Instense light bursts in the stimulated Raman effect,” Phys. Rev. Lett. 17(26), 1275–1277 (1966).

28. M. Maier, W. Kaiser, and J. A. Giordmaine, “Backward stimulated Raman scattering,” Phys. Rev. 177(2), 580–599 (1969).

29. P. L. Kelley and T. K. Gustafson, “Backward stimulated light scattering and the limiting diameters of self-focussed light beams,” Phys. Rev. A 8(1), 315–318 (1973).

30. R. R. Alfano and G. A. Zawadzkas, “Observation of backward-stimulated Raman scattering generated by laser pulses in liquids,” Phys. Rev. A 9(2), 822–824 (1974).

31. J. Ren, W. Cheng, S. Li, and S. Suckewer, “A new method for generating ultraintense and ultrashort laser pulses,” Nat. Phys. 3(10), 732–736 (2007).

32. S. V. Kurbasov and L. L. Losev, “Raman compression of picosecond microjoule laser pulses in KGd(WO4)2 crystal,” Opt. Commun. 168(1-4), 227–232 (1999).

33. C. Canalias and V. Pasiskevicius, “Mirrorless optical parametric oscillator,” Nat. Photonics 1(8), 459–462 (2007).

34. G. Strömqvist, V. Pasiskevicius, C. Canalias, and C. Montes, “Coherent phase-modulation transfer in counterpropagating parametric down-conversion,” Phys. Rev. A 84(2), 023825 (2011).

35. G. E. Kugel, F. Bréhat, B. Wyncke, M. D. Fontana, G. Marnier, C. Carabatos-Nedlec, and J. Mangin, “The vibrational spectrum of a KTiOPO4, single crystal studied by Raman and infrared reflectivity spectroscopy,” J. Phys. C Solid State Phys. 21(32), 5565–5583 (1988).

36. V. Pasiskevicius, A. Fragemann, F. Laurell, R. Butkus, V. Smilgevicius, and A. Piskarskas, “Enhanced stimulated Raman scattering in optical parametric oscillators from periodically poled KTiOPO4,” Appl. Phys. Lett. 82(3), 325–327 (2003).

37. S. E. Harris, “Proposed backward wave oscillation in the infrared,” Appl. Phys. Lett. 9(3), 114–116 (1966). 38. M. G. Raymer, J. Mostowski, and J. L. Carlsten, “Theory of stimulated Raman scattering with broad-band

lasers,” Phys. Rev. A 19(6), 2304–2316 (1979). 39. D. D. Lowenthal, “CW periodically poled LiNbO3 optical parametricoscillator model with strong idler

absorption,” IEEE J. Quantum Electron. 34(8), 1356–1366 (1998). 40. M. M. Fejer, G. A. Magel, D. H. Jundt, and R. L. Byer, “Quasi-Phase-Matched second harmonic generation -

tuning and tolerances,” IEEE J. Quantum Electron. 28(11), 2631–2654 (1992).

1. Introduction

KTiOPO4 (KTP) and its isomorphs are well-established ferroelectric nonlinear optical materials used for second-order frequency conversion applications. Electric-field poling can be used in these crystals to tailor the spatial profile of the effective nonlinear coefficient to produce quasi-phase matched (QPM) structures. Similar to other ferroelectrics, e.g. LiNbO3 and LiTaO3, KTP is characterized by strong coupling of terahertz (THz) electromagnetic waves to the mechanical degrees of freedom, i.e. the transversal optical (TO) phonon modes, which gives rise to a very efficient phonon-polariton scattering [1–5]. The TO phonon modes


involved in the polariton excitation are infrared-active with concomitant emergence of absorption for larger polariton wave-vectors. In ferroelectrics, most of these TO lattice vibrations are also Raman-active, although it is not a requirement for realizing polariton coupling [5,6]. The second-order nonlinearity, χ(2), can have a large dispersion in the polariton frequency range [1,7–10]. Due to the coherent superposition of the non-resonant electronic contribution with the polar lattice vibrations, the overall χ(2) can be enhanced (or reduced) in the spectral regions around the TO vibrational modes. In general, stimulated polariton scattering (SPS) involves both the second-order and third-order, Raman, nonlinearities [1,11,12]. As well as those previously reported in LiNbO3 [13], efficient forward SPS (FSPS) with a small wave-vector of polaritons is behind the recent demonstrations of tunable THz nanosecond optical parametric oscillators in a single-domain KTP [14] and KTiOAsO4 [15]. Coherence and relatively low absorption of small-k polariton waves generated in FSPS opened up possibilities for demonstration of polaritonic photonic crystals, waveguides and other intriguing opportunities for their use in on-chip THz applications [16–18].

The response times of the χ(2) associated with the strongest TO phonons are of the order of 1 ps in KTP [4], which is much slower than the non-resonant electronic part of the nonlinearity. For instance, in THz generation employing optical rectification of near-infrared femtosecond pulses in QPM ferroelectrics [19–22], it is mostly the electronic part of χ(2) that is harnessed due to the short excitation pulses. In such situation, coupling to other mechanical degrees of freedom in the lattice can also happen through an impulse generation of coherent phonons, which has been observed in various solid state materials [23,24]. It is tempting to think that, for pulses longer than the characteristic response time of the lattice dipoles, one could exploit the flexibility afforded by the QPM techniques and, at the same time, harness the enhanced χ(2) nonlinearity offered by the lattice dipole system. However, we have recently demonstrated that FSPS with such long pump pulses is strongly suppressed in periodically-poled KTP (PPKTP) [12]. The FSPS suppression results from the interplay between the third-order Raman and the second-order nonlinearities associated with the same TO phonons, which results in the generation of antiphase polariton waves in adjacent ferroelectric domains and, therefore, leads to parametric de-amplification of the THz wave. Recent reports on THz generation in OPOs using periodically poled Mg:LiNbO3 (PPLN) pumped with nanosecond pulses seem to show that, at least to some extent, similar suppression of the polariton generation takes place in this material as well [25,26].

In this work, we show that a rather surprising corollary of the FSPS suppression in PPKTP is a strong enhancement of backward SPS (BSPS). The observed BSPS is highly efficient with more than 50% of the pump energy being transferred to the backwards propagating Stokes. Moreover, as in backward Stimulated Raman scattering (BSRS), the Stokes pulses generated in BSPS also experience substantial compression in time domain. Superficially, BSPS bares certain similarities to BSRS, which was first observed in a CS2 liquid in 1966 [27]. The signature of the BSRS as observed in long liquid cells (typically tens of cm long) is the generation of intense Stokes pulses in the backward direction with a pulse length much shorter than that of the pump [28]. However, BSRS requires relatively high intensities to become efficient, since forward scattering first takes place in most cases. Due to inherent symmetry in the stimulated Raman scattering, the backward and forward scattering cannot be disassociated, i.e., both processes happen at the same time. Although BSRS was proposed as a mechanism limiting beam radius in filaments under self-focusing conditions [29,30], and also as means for high-intensity ultrashort pulse generation in plasmas [31], the requirement for high pump intensity that is close to the optical damage threshold makes it rather difficult to utilize the backward stimulated Raman process in crystals [32]. In contrast to BSRS, however, the BSPS process in PPKTP can be well separated from the forward polariton scattering. We show here that the threshold and efficiency of the BSPS process in PPKTP is far below self-focusing or optical damage threshold. In fact, BSPS can be a strong competing process in counter-propagating QPM optical parametric devices [33,34].


2. Backward

The energy c

conditions arethe indices, s,diagrams for tdispersive wacollinearly. Frwave-vector i

where sϕ is t

vectors as shpolarization ppolariton coup

Figure 1(dispersion curpolariton dispwhere we usethe phonon dathe TO and thabsorption spresonances, tconfiguration the experimenthe pump wav

(1) using th

1.8 ,3.4sϕ =

The intersectmatching poin

Fig. 1observabsorplines) polari

angles

singleperiod

d stimulated

conservation, ωe satisfied in S p, pol, denote the FSPS and Baves, the forwarom the momeis given by:

the internal an

hown in Fig. 1parallel to thepling arises frob) compares rve and the co

persion calculaed the Lorentzata from [35]. The associated Lectra owing to the polariton of FSPS in a

ntal data that cvelength of 80

he fixed wave , correspondin

tion of these nts in good agr

1. (a) The phase-mved in single-domption spectrum (blphonons used to

iton wave-vectors

s 0 ,1 .8sϕ = °e-domain KTP (bdicity.

polariton sc

s p polω ω ω= −SPS. Here, ωStokes, pump

BSPS processeard scattering entum conserva

2

pol p=k k

ngle between

1(a). For the pe crystal z-axisom A1 symmetthe phase-mat

orresponding abted by taking i

zian series reprThe dashed blaLO phonons, wthese infrareddispersion stsingle-domain

corresponds to07 nm. The red

e-vector p =k

ng to the exper

curves with threement with th

matching conditionmain KTP. (b) Plue line). Frequenmodel polariton calculated from E

8 , 3.4 ,1 80° ° °lue dots) [12], an

cattering

, and the mo

is the cyclic fand polariton

es are shown ingenerates the ation, it follow

22s p+ −k k

the directions

pump propagats, i.e. in the Xtry TO phonontched FSPS absorption specinto account teresentation of ack and red linwhereas the sold-active TO photrongly dictaten KTP [12,36].o the polaritond lines in this

31.44 10= × cm

rimentally mea

he polariton dhe experiment.

ns for FSPS and Polariton dispersioncies of TO (blackdispersion and ab

Eq. (1) for the fixe

. Polaritons obse

nd BSPS in PPK

omentum conse

frequency, k iwaves, respect

n Fig. 1(a). SinStokes and th

ws that the mag

coss sϕk

of the pump

ting along theX(ZZ)X confi

ns. and BSPS mactrum. The blaen strongest TOthe complex d

nes represent thlid blue line reonons. In the ves the noncol. The blue dots generated infigure have be

m−1 at 807 n

asured internal

dispersion giv

BSPS. Only non-on in KTP (blackk dashed lines) anbsorption. Red soled pump waveleng

erved experiment

KTP (green dots)

ervation s =k

is the wave-vetively. The wav

nce polaritons ae polariton wagnitude of the

and the Stok

e crystal x-axisiguration, the

arked on the ack solid line sO phonon linesdielectric func

he central frequepresents the cvicinity of thesllinear phase-ts in Fig. 1(b) n the FSPS proeen calculated

nm and the

l Stokes angles

ves the expect

-collinear FSPS isk solid line) and

nd LO (red dashedlid lines representgth of 807 nm and

tally in FSPS in

with e.g. 36 µm

p pol−k k

ector, and ve-vector

are highly aves non-polariton

(1)

kes wave-

s and the strongest

polariton shows the s in KTP, ction with uencies of calculated se phonon matching represent

ocesses at from Eq.

angle of

s in KTP.

ted phase

s d d t d

n

m


In the case of BSPS, the Stokes wave is generated in opposite direction to the pump, 180sϕ = , as described in Fig. 1(a). Therefore, the momentum conservation,

pol p s= +k k k , requires a large polariton wave-vector, i.e. 2pol p≈k k . The required

polk as a function of frequency in the BSPS process was calculated from Eq. (1) and shown

by the red solid line marked 180sϕ = in Fig. 1(b). The green data points mark the polariton

frequencies observed in our experiment. In this range of large momenta, the polariton dispersion is rather flat and asymptotically approaching to a TO phonon frequency responsible for that particular polariton branch till the Brillouin zone boundary. In this case, the refractive index of the polaritons generated in BSPS can be very large, namely:

( ) ppol p s s

pol

n n n nωω

= + − (2)

where ns, np are refractive indices of the Stokes and the pump, respectively. The values of the indices of refraction and other parameters for the polaritons at the green data points in Fig. 1(b) are given in the Table 1.

Table 1. Parameters of the polaritons observed in backward stimulated polariton scattering (BSPS) in PPKTP with e.g. 36 µm periodicity.

fpol [THz] λpol [nm] npol kpol [104 cm−1] 1/α [µm] 5.5 220 247 28.5 47

8 221 169 28.4 0.5

20.6 225 65 27.9 1 fpol: Stokes Shift, λpol: Polariton Wavelength in the crystal, npol: Index of refraction, kpol: Wave-vector, 1/α: Absorption length.

Please note that the phase-matching condition for BSPS in PPKTP does not involve the grating vector in the equation. This is because the slow polariton waves do not experience the poling periods before the absorption takes over. Large absorption of the polaritons would limit the effective interaction length to about 1 µm for the strongest polariton lines in BSPS (8 THz and 20.6 THz), which corresponds to only few polariton wavelengths in the crystal. This also renders the above-mentioned suppression mechanism of polariton scattering inefficient in PPKTP in the backward-propagating geometry. Instead, as presented below, it is observed that BSPS gets strongly enhanced in PPKTP with the phase-matching condition independent of the poling periods.

3. Experimental results and discussion

In order to study the effect of (2)χ structuring on the BSPS threshold, we compared single-

domain KTP crystals with several PPKTP structures with different periodicities ranging from 9 µm to 500 µm. All the crystals had the same crystal length of 11.6 mm, which was fully covered by each grating. As a pump source, we used a picosecond Ti:Sapphire regenerative amplifier operating at 807 nm with a pulse spectral bandwidth of 0.7 nm to produce the pulse length tunable from 1.5 ps to about 200 ps by adjusting dispersion in the amplifier. BSPS was observed in the X(ZZ)X configuration, i.e. with the pump beam propagating along the crystal

x-axis and polarization parallel to the crystal z-axis. The PPKTP structures were slightly tilted to prevent Fresnel reflections from interfering with the measurements. In this configuration, it was verified that the BSPS Stokes beam is generated in the counter-propagating direction to the pump. Figure 2(a) shows the measured BSPS threshold as a function of poling period in PPKTP. As the poling period becomes smaller, FSPS is increasingly suppressed [12], eventually leaving BSPS the dominant polariton scattering process in PPKTP with the 9 µm period. In the PPKTP crystals with long periodicities, the BSPS threshold approaches that of


the single-domain KTP. In these crystals, the BSPS has substantially higher pump threshold compared to the FSPS, consequently making the BSPS process inefficient. Two dominant polariton lines, 8 THz and 20.6 THz, have been observed in BSPS for all crystals, which is shown in Fig. 2(b). The frequency of the polaritons giving rise to BSPS did not depend on the poling period. For the crystals with periodicities below 36 µm, where BSPS is already dominant, a new and weaker polariton line at 5.5 THz starts to emerge. We tentatively attribute it to 6.1 THz TO phonon, which has relatively low oscillator strength [35] compared with much stronger vibrations at 8.04 THz and 21 THz.

Fig. 2. (a) The observed intensity-thresholds of BSPS as a function of poling period with a fixed pump pulse duration of 47 ps. The error bars stem primarily from the uncertainty in beam-size measurements. (b) The pump at 807 nm and the observed BSPS spectrum associated with the TO phonon lines in PPKTP with the poling period of 36 µm. The amplitudes of the 5.5 THz and 8 THz are suppressed with respect to 21 THz line due to lower reflectivity of the beam-splitter in front of the PPKTP crystal. The Fresnel reflection of the pump propagates in a slightly different direction owing to intentional tilting of the crystal.

Fig. 3. (a) Pump depletion and the corresponding BSPS efficiency as a function of pump intensity with a fixed pump pulse duration of 200 ps in PPKTP with the periodicity of 9 µm. (b) The measured dependence of the BSPS threshold on the pump pulse length for the Stokes at 8 THz (red squares) and 20.6 THz (blue squares). Blue and red lines represent power fits to the measured data. The black solid line represents inverse square dependence, which is expected in lossless counter-propagating parametric oscillator. The PPKTP structure with the periodicity of 9 µm was used in these measurements.

According to Fermi’s golden rule, the SPS coupling efficiency associated with a particular TO phonon mode would depend on the density of polariton states. The spectrum of the density of states (DOS) can be estimated from polariton dispersion via the Hilbert transform

of ( )22 /pol polk kπ ω∂ ∂ . The ratio of the normalized DOS to the normalized absorption at the

phase-matched polariton frequency can be used as a “figure of merit” that indicates the expected net gain for each polariton mode. These ratios for the polaritons responsible for BSPS at 5.5 THz, 8 THz and 20.06 THz are respectively 0.508, 1.6, and 0.823. Therefore, it


is expected this confirmed i

We emphatotally suppreintensity ~3 pumped with forward-propapower transfewhere the baprocesses. Ththree-wave moscillation (Mthe square ointeraction le

experimental function on tTHz and 20.

proportional t

is the laser puthe laser puls

and 21 THz respectively, w

Fig. 4In (a)(soliddenotesolid l

One of thsubstantially sindication of the non-phasehigher than thpulse length othat was compreference pumin a type-I phthrough a diseparation of cross-correlat

hat BSPS involin our experimasize that the Bessed. As showtimes the thre200 ps-long p

agating paramer from the puackward scatterhis behavior o

mixing throughMOPO) [33,37]

f the pump pength /L cτ=data in Fig. 3(he pump puls6 THz, respec

to ( )TO L

−Γ + Γulse bandwidthe length τ , pr

would suppowhich are subs

4. Cross-correlation, squares denote Sblack: 2.2 GW/cm

e Stokes correspolines represent Gau

he signatures oshorter than tha high-peak ine matched secohat produced bof the backwarpressed to the t

mp after passinghase-matched Biffraction gratithe sum-frequ

tion traces of th

lving 8 THz poments with diffeBSPS process iwn in Fig. 3(a)eshold. Here, pulses. In such etric processesump. This is iring is relative

of the BSPS ph χ(2) nonlinear]. The oscillatipulse length, τ(2 )pn shorter

(b) shows that e length, althoctively. In con1

[38], where

h. Therefore, trovided that TΓort the transfostantially shorte

n measurements foStokes correspondm2, solid blue: 4.7nding to 21 THz ussian fits.

f the BSRS ishe pump pulsesntensity in the Sond harmonic by the forward rd Stokes via crtransform-limig through a va

BBO crystal. Ting onto a Si

uency fields stehe backward St

olaritons woulderent PPKTP sais very efficien), the efficiencthe PPKTP ssituations, the

s, which makein total contraely inefficient

process bears srity that gives ion threshold i

2τ − , providedthan that of

BSPS threshoough it scales ntrast to BSPS

TOΓ is the spo

he gain in BSR1TOτ >> . The

orm-limited Gaer than the pum

or backward propading to 8 THz pola GW/cm2, open blpolaritons at the p

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ross-correlatioted length of 1

ariable delay linThe resulting sui p-i-n photodemming from ttokes at differe

d have the lowamples. nt in PPKTP stcy of BSPS reastructure with ere is no quasi-es BSPS extremast to BSRS, th

due to dominsimilarities wirise to mirror

in MOPO is ind that the pulf the crystal.

old also dependas 1.62τ − and τ

S and MOPO

ontaneous Ram

RS should be bandwidths of

aussian pulsesmp pulses used

agating Stokes (a) aritons at differenlack: 11 GW/cm2)pump intensity of

n of intense Sur BSPS experitially came frothe backward dpump. We subson with a small1.5 ps. The Stokne were superimum-frequency detector, wherthe Stokes at 8ent pump inten

west threshold,

tructures whereaches 70% at t9 µm periodi

-phase matchinmely efficient the third ordernant forward sith counter-prorless optical pnversely propolses have the Indeed, the f

ds on the inver1.73τ − for the B

, the gain in

man bandwidth

largely indepef TO modes at

s of 2 ps andd in our experim

and the pump (b)nt pump intensities), while red circlesf 11 GW/cm2. Red

Stokes spikes wriment with PPom the observdirection was msequently meal part of the pukes and the composed non-cogeneration wa

re the grating8 THz and 21 Tnsities are show

as indeed

e FSPS is the pump icity was ng of any with full

r process, scattering opagating arametric

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fit to the

rse power BSPS at 8

BSRS is

h and LΓ

endent on t 8.1 THz

d 0.8 ps, ments.

. s s d

which are PKTP, the ation that markedly

asured the ump pulse mpressed ollinearly as imaged g enabled THz. The wn in Fig.


4(a), while that of the incoming pump is displayed in Fig. 4(b). The pulse shape of the backward propagating wave depended strongly on the pump intensity above the threshold. The general tendencies can be observed in the traces of the 8 THz Stokes. Just above the threshold, the pulse is a well-defined Gaussian with the FWHM of about 19 ps. As the pump intensity is increased up to 4.7 GW/cm2, the backward Stokes pulse acquires a double-peak structure which could be fit with a sum of two Gaussian pulses, one centered at 47 ps with the FWHM of 41 ps, and the other at 82 ps with the FWHM of 9 ps. Similar structure, albeit more compressed in time, is retained at the highest pump intensity of 11 GW/cm2. The backward Stokes pulse corresponding to the 20.6 THz polaritons always had a single-Gaussian shape, which was centered at 45 ps with the FWHM of 22 ps at the highest pump intensity.

Fig. 5. Calculated normalized stationary signal (Stokes, blue lines) and idler (polariton, red lines) intensity distributions for different values of polariton absorption coefficient. The arrows indicate the directions of propagation for each wave. Pump intensity of 13 GW/cm2 is used in the calculations with the effective nonlinear coefficient of 183 pm/V [12]. The intensity distributions give increasingly shorter amplification lengths as the absorption increases. Note that the absorption coefficient of 40 cm−1 already limits the parametric gain region at the beginning of the crystal. The actual polariton absorption coefficient involved in BSPS is as large as 10 4 cm−1 as previously shown in Table 1.

The change in the pulse shape indicates that the BSPS is not a stationary process, which differs from the near-infrared counter-propagating parametric oscillators. This difference is ascribed to the fact that the absorption of the polariton wave generated in BSPS is very large, as shown in Table 1. The role of the large polariton absorption in the counter-propagating geometry is shown in Fig. 5 by calculating the normalized intensity distributions of polaritons and Stokes along the crystal. The results were obtained by numerically solving coupled-wave equations with second-order nonlinear interaction of monochromatic waves in counter-propagating geometry [39]. As the absorption of the polariton wave is increased, the parametric gain region is increasingly concentrated at the beginning of the crystal. The intensity buildup in Stokes field, however, is not achieved immediately. One can estimate the time-scale of the Stokes intensity buildup as gp gs(v v )cL + , where Lc is the crystal length, and

vgp, vgs are the group velocities of the pump and the signal, respectively. For the crystals used in our experiment, this time scale is about 40 ps, which generally agrees with the position of the first intensity peaks in the Stokes cross-correlation traces. The Stokes and polariton buildup strongly depletes downstream pump, which leads to a self-termination of the process as the first Stokes pulse exits the crystal. At higher pump intensities, however, the buildup process can repeat itself, but on a shorter temporal scale, as some parametric gain is still present at the beginning of the crystal. This second pulse then should be shorter and more intense. This qualitative picture explains the experimental observations. It should be noted that BSRS would also result in multiple pulsing if the length of the gain medium is shorter than the optical length of the pump pulse. However, the Stokes pulse in BSRS should be


strongly asymmetric with the leading edge of the pulse being much steeper, since the backward Stokes pulse continuously encounters the undepleted part of the pump as it sweeps through it [28].

As already shown, the BSPS process can become a very efficient and dominant one in PPKTP. The process can be used in a number of applications where a high peak intensity or a frequency-shifted beam in the direction conjugate to the pump is required. On the other hand, in circumstances with near- and mid-infrared parametric QPM devices, the BSPS might be detrimental. In a good-quality PPKTP structures where other processes are phase-matched, the BSPS is usually not observed due to the pump depletion before the BSPS can reach its threshold. However, fabrication of QPM structures can impart errors to the periodicity in the structures, or to the duty cycle of ferroelectric domains. Therefore, it is instructive to estimate the error margin above which the BSPS is expected to become a competing nonlinear process. This is especially important for QPM structures with sub-micrometer periodicity, which is used in mirrorless OPOs and other counter-propagating parametric frequency converters. The product of the parametric gain and the interaction length gL has the same functional form for

the BSPS and the near-infrared parametric devices:

( )2 2

2 eff

s i s i

d LgL

n n λ λ∝ (3)

where deff, ns, ni, λs, λi, are, respectively, the effective nonlinear coefficient, the refractive indices of the signal (Stokes in BSPS) and the idler (polariton in BSPS), the wavelengths of the signal and the idler. The nonlinear coupling for BSPS can be quite large, owing to the large effective nonlinear coefficient in the vicinity of polariton resonances [12]. Taking a specific example of the PPKTP MOPO pumped at 800 nm, generating the signal, λs = 1.18

µm, and the idler λi = 2.9 µm, we get ( )2 2 2 28.9 /NIR NIR NIRg L L pm V ∝ . Here, LNIR is

measured in microns, and represents the effective length of the QPM structure, which might be different from the physical length of the QPM structure due to fabrication errors. For the

BSPS process, we have ( )2 2 2 23.5 /polg L L pm V ∝ where L is now the physical length of

the QPM structure. As clarified above, the slow polariton wave will not move appreciably before being absorbed. Therefore, the errors in the domain periodicity are irrelevant to the efficiency of the BSPS process. From this estimate, it is clear that the near- or mid-infrared parametric QPM process in PPKTP will always have lower threshold than that of BSPS in a perfect QPM structure with no errors. However, both processes will have equal gain if the effective QPM length is 38% shorter than the physical length of the structure, provided that the QPM errors are uniformly distributed over the physical structure. For example, if we consider the asymmetry in the duty cycle, which is one of the most common fabrication errors encountered in sub-micrometer periodicity structures, this error will reduce the effective nonlinearity deff for the near-infrared parametric process [40]. In this case, the BSPS will have equal gain with the near-infrared parametric process when the duty cycle is reduced from the perfect 0.5 to about 0.22. For such imperfect structures, there is a high probability that the BSPS will become efficient and prevent counter-propagating parametric oscillation in near- and mid-infrared.

4. Conclusions

In conclusion, we have shown a rather surprising dominance of the BSPS process in PPKTP structures, where it was possible to convert 70% of pump power into Stokes propagating in the backward direction. The suppression of the forward polariton scattering in the χ(2) structures with periodicity smaller than about 36 µm makes the BSPS very efficient, owing to the strong enhancement of the effective second-order nonlinearity near the phonon-polariton


resonances. The enhancement is most prominent for the pump pulses longer than the inverse bandwidth of the TO-phonon modes that are responsible for the polariton branches. BSPS can be understood primarily as a second-order parametric process in counter-propagating geometry, although this does not preclude a role of third-order Raman scattering in the same crystals. The BSPS is essentially a non-stationary process where the backwards generated Stokes is comprised of pulses with the shape dependent on the pump intensity. This includes a substantial pulse compression with higher peak intensity compared with the pump. There are certain superficial similarities between BSPS and BSRS, which can be surprising if one considers that SRS is produced by localized dispersionless lattice optical phonons whose phase is essentially irrelevant for the SRS outcome. In general, the relative phases of the interacting waves in the second-order parametric process play an important role in the phase-matching condition. In BSPS, however, the polariton wave is extremely slow and strongly absorbed such that the phase information cannot be transferred so far. Therefore, the polariton phase will be dictated by the interaction of the counter-propagating pump and Stokes. In principle, this physical mechanism is rather general and should not be limited to KTP and its isomorphs.

Acknowledgments

We would like to acknowledge the Swedish Research Council (VR), Linné Center ADOPT, and Göran Gustafsson Foundation, and Swedish Foundation for Strategic Research for financial support of this work.


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