## Abstract

We study second harmonic generation in a 2-D photonic crystal with the pump field tuned at the Dirac point of the structure. The simultaneous generation of both forward and backward phase-matched second harmonic is achieved by exploiting a peculiar regime in which the interacting waves have zero phase velocity in the lattice. This regime can be attained even when strong material dispersion is present and therefore lends itself well to be implemented in semiconductor-based frequency conversion devices. A comparison between this method and the quasi-phase-matching technique is also presented.

© 2014 Optical Society of America

## 1. Introduction

Increasing the coherence length of frequency conversion processes has always been one of the main objectives in the field of nonlinear optics since the experiment of *Franken* and associates [1] in which an extremely small fraction of photons of a ruby laser beam (694 nm) was converted into ultraviolet light (347 nm) at twice the frequency, after the beam was propagated through a quartz crystal. It was soon realized that the poor conversion efficiency had to be ascribed to the normal material dispersion which caused the fundamental and second harmonic waves to travel along the crystal with different phase velocities. Under these circumstances, the second harmonic (SH) field radiated by the oscillating dipoles induced by the fundamental frequency (FF) field can add together constructively only over the coherence length l_{c} = π/∣Δk∣, where Δk = (2ω/c)(n_{2ω}-n_{ω}) is the momentum mismatch (or phase mismatch), n_{ω} and n_{2ω} are respectively the refractive index of the material at the FF and SH. Shortly after Franken and associates experiment [1], *Giordamaine* [2] and *Maker et al.* [3] simultaneously proposed a way to match the phase velocities of the waves at the FF and SH based on the anisotropy properties of certain birefringent crystals, such as potassium dihydrogen phosphate (KDP). The use of birefringent crystals is the most common method to achieve phase matching. More recently, another technique, quasi-phase-matching (QPM), has become extensively utilized [4]. In the QPM approach the correction to the relative phase mismatch between the FF and SH is achieved by periodically alternating the domains of the quadratic nonlinearity. Harmonic generation has also been examined in epsilon-near-zero materials during the past [5,6] and recent [7–9] years. Another approach to achieve phase matching is offered by photonic crystals. Photonic crystals (PCs) or photonic band gap structures (PBGs) [10–14] can in general be described as structures in which a periodic variation of the linear refractive index of the medium in 1-D, 2-D or 3-D gives rise to allowed and forbidden band for photons in essentially the same way that semiconductors do for electrons. For the FF and SH waves interacting in the periodic lattice, the momentum mismatch can be compensated by the reciprocal lattice vectors of the crystal itself as:

## 2. Results and discussion

In Fig. 1 we show the PC structure studied.

In Fig. 2 we show the photonic band gap structure of the infinitely periodic lattice with d*/*a *=* 0.35. The structure admits a Dirac point at ωa/2πc≅0.53 on the Γ point (i.e. for normal incidence). Two branches of linear dispersion intersect at the Γ point, an additional flat branch is also present corresponding to quasi-longitudinal modes. This sort of topological dispersion around the Dirac point is quite common not only for 2-D square lattices [27], but also for different lattice arrangements, such as the triangular lattice [28]. For computational speed we have used square columns but similar results can be obtained for circular columns as well.

The simplest way to achieve phase matching in such kinds of structures is to tune the FF on the Γ point corresponding to the Dirac point and allow the SH to be generated on another Γ point (as shown in Fig. 2). This way, the Bloch vector of both FF and SH is zero modulus one of the reciprocal lattice vectors and simultaneous forward and backward phase matching can be achieved according to Eq. (1). In this particular case, we have considered the columns to be made of a linearly dispersive material with refractive index at the FF and SH respectively n_{ω}≅3.62 and n_{2ω}≅3.82. Those values are in the range of the dispersion in the visible and near-IR of several semiconductor materials [31], for example GaAs has a refractive index of ~3.4 at 1.8μm and ~3.6 at 0.9μm. While here we do not refer to a specific material in particular, nonetheless we mention that the alignment of the SH at the Γ point may be sought by properly tailoring the geometrical characteristics of the PC, i.e. d*/*a (or r/a in the case of circular columns) and/or the lattice arrangement, so to compensate the dispersion of the specific material under consideration on a case by case basis.

In Fig. 2 we have superimposed the transmittance, i.e. transmitted power divided incident power, of a finite N = 10 period structure onto the photonic band structure of the infinitely periodic lattice. It is noted that the Dirac point is exactly located at the center of the second pass band of the finite structure at normal incidence. The numerical calculation of the transmittance has been performed using an in-house developed code based on the Fourier-modal-method (FMM) [32]. The calculation of the Bloch dispersion has been performed by using another in-house developed code that finds the unitary amplitude complex eigenvalues of the transfer matrix according to the recipe laid out in [33]. In Fig. 3 we highlight the tuning conditions of the FF and SH on the dispersion of the infinitely periodic lattice (3(a) and 3(c)) and on the transmittance of the finite 10-period structure (3(b) and 3(d)).

The perfect phase matching condition is achieved when the second harmonic is tuned at the band edge. The band edge is always in the region where the transmittance decreases as it approaches the band gap and it should not be confused with the spectral position of the band edge transmission resonance. In this paper we are not exploiting a double resonant condition, i.e the case in which the FF and SH are both tuned on transmission resonances of the structure. In other words, we do not rely on the enhancement of the density of modes at the FF and SH, but we are instead exploring a true phase matching condition where, as we will see in a moment, the conversion efficiency increases as the square of the length of the structure.

In order to confirm the results of the previous analysis, we have calculated the SH conversion efficiency for three topical cases, as exemplified in Fig. 4.

First we consider the conversion efficiency (generated SH power divided incident FF power) of a non-phase-matched bulk medium having a quadratic nonlinearity over a length L, then we consider the conversion efficiency from the same bulk of length L where the QPM technique has been used to compensate the phase mismatch, and, finally, we study the conversion efficiency of the 2-D PC made of the same material and same total length L under the tuning conditions previously elucidated. In the comparison we use the first order QPM, i.e. we periodically invert the sign of the quadratic domains each coherence length [4]. In particular, we have considered two sub-cases: the QPM for the compensation of the phase mismatch of the forward generated SH and the one for the compensation of the phase mismatch of the backward generated SH. Note that the compensation of the phase mismatch of the backward SH is more difficult to achieve experimentally [4] because backward SH coherence length is much smaller than forward SH coherence length and requires an inversion of the sign of the domains on short distances. On the contrary, in the case of the PC, the particular tuning conditions previously reported, i.e. the FF and SH aligned at the Γ point, make possible the simultaneous phase matching of both the forward the backward SH. The conversion efficiency has been calculated by a straightforward extension to 2-D structures of the coupled mode theory for quadratic interactions previously developed for 1-D structures [34]. The results of the calculation are reported in Fig. 5 and Fig. 6 for a value of the quadratic nonlinearity d^{(2)} = 9pm/V, an input intensity of 100MW/cm^{2}, and forward coherence length of the bulk material of ~2a.

Figures 5 and 6 show how the conversion efficiency for the PC scales exactly as L^{2}. This is a clear indication that the generation is happening under perfect phase matching conditions, in agreement with the previous analysis based on the Bloch dispersion. Moreover the backward and forward generated SH are perfectly balanced [35] and the total conversion efficiency (forward + backward) roughly equals the one that is obtained by the QPM technique. If just the forward conversion efficiency is detected, the QPM gives roughly double the conversion efficiency. The comparison with the backward QPM is more a scholastic than a practical case, given the extremely short coherence length of the backward SH which would require an inversion of the quadratic domains over exceptionally small distances. In this sense the phase matched backward generated SH from the PC represents a truly remarkable result. It is even more significant if we consider that the filling fraction of the quadratic material in the PC is only 10% compared to the 100% in the QPM case. Finally in Fig. 7 we show a snapshot of the FF pump field tuned at the Dirac point and the SH generated field for the 10-period structure. For an animation of the time evolution of the fields see Media 1.

The animation shows how at the Dirac point the photonic crystal basically acts as perfect transparent material, the wave-front of the incident FF field undergoes minimal distortion as it propagates through the crystal and it is completely transmitted, in agreement with previous studies [29]. It is also noted that the SH field is indeed generated perfectly balanced in the forward and backward direction, as one may expect based on the Bloch vector analysis. We have also performed additional calculations for the conversion efficiency when the SH field is slightly misaligned with respect to the Γ point and found that, as expected, the conversion efficiency roughly scales as: sinc^{2}(ΔK_{β}L/2) where ΔK_{β} is the Bloch vector mismatch.

## 3. Conclusions

In conclusion, we have studied phase matched SH generation with the pump field tuned at the Dirac-point of a 2-D photonic crystal. We have shown that perfectly balanced, phase-matched SH emission can be achieved when the SH is aligned at a Γ point of the structure. This procedure can be compatible with the dispersion characteristics of several semiconductor materials by properly tailoring the geometrical characteristics of the PC. Although here we have focused on a square lattice with square columns, similar results can be obtained for different lattice arrangements and/or different shapes of the columns. Moreover, while here we have concentrated our attention on the coupling with both the FF and SH fields polarized parallel to the columns, different coupling conditions can be explored as well, depending on the particular symmetry properties of the quadratic tensor of the material employed. In general, we expect similar results provided that the alignment of the pump and the generated SH respectively at the Dirac point and at the Γ point is attainable. The concepts elucidated in the present work could also be extended to parametric interactions, such as three-wave mixing, with the pump field tuned at the Dirac point and the idler and signal aligned at two Γ points opening new scenarios in the field of nonlinear frequency conversion devices.

## Acknowledgments

This work has been supported by DARPA SBIR project number W31P4Q-11-C-0109.

## References and links

**1. **P. A. Franken, A. E. Hill, C. W. Peters, and G. Weinreich, “Generation of Optical Harmonics,” Phys. Rev. Lett. **7**(4), 118–119 (1961). [CrossRef]

**2. **J. A. Giordmaine, “Mixing of Light Beams in Crystals,” Phys. Rev. Lett. **8**(1), 19–20 (1962). [CrossRef]

**3. **P. D. Maker, R. W. Terhune, M. Nisenoff, and C. M. Savage, “Effects of Dispersion and Focusing on the Production of Optical Harmonics,” Phys. Rev. Lett. **8**(1), 21–22 (1962). [CrossRef]

**4. **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). [CrossRef]

**5. **G. D’Aguanno, N. Mattiucci, M. J. Bloemer, and M. Scalora, “Large Enhancement of Interface Second-Harmonic Generation Near the Zero-n Gap of a Negative-Index Bragg Grating,” Phys. Rev. E Stat. Nonlin. Soft Matter Phys. **73**(3), 036603 (2006). [CrossRef]

**6. **G. D’Aguanno, N. Mattiucci, M. Scalora, and M. J. Bloemer, “Second-Harmonic Generation at Angular Incidence in a Negative-Positive Index Photonic Band-Gap Structure,” Phys. Rev. E Stat. Nonlin. Soft Matter Phys. **74**(2), 026608 (2006). [CrossRef]

**7. **M. A. Vincenti, D. de Ceglia, J. W. Haus, and M. Scalora, “Harmonic generation in multiresonant plasma films,” Phys. Rev. A **88**(4), 043812 (2013). [CrossRef]

**8. **D. de Ceglia, S. Campione, M. A. Vincenti, F. Capolino, and M. Scalora, “Low-damping epsilon-near-zero slabs: Nonlinear and nonlocal optical properties,” Phys. Rev. B **87**(15), 155140 (2013). [CrossRef]

**9. **H. Suchowski, K. O’Brien, Z. J. Wong, A. Salandrino, X. Yin, and X. Zhang, “Phase Mismatch-Free Nonlinear Propagation in Optical Zero-Index Materials,” Science **342**(6163), 1223–1226 (2013). [CrossRef]

**10. **E. Yablonovitch, “Inhibited spontaneous emission in solid-state physics and electronics,” Phys. Rev. Lett. **58**(20), 2059–2062 (1987). [CrossRef]

**11. **S. John, “Strong localization of photons in certain disordered dielectric superlattices,” Phys. Rev. Lett. **58**(23), 2486–2489 (1987). [CrossRef]

**12. **J. D. Joannopoulos, R. D. Meade, and J. N. Winn, *Photonic Crystals, Molding the Flow of Light.* (Princeton University, 1995).

**13. **J. M. Lourtioz, H. Benisty, V. Berger, J.-M. Gérard, D. Maystre, and A. Tchelnokov, *Photonic Crystals*, (Springer, 2005).

**14. **Y. S. Kivshar and G. P. Agrawal, *Optical Solitons: From Fibers to Photonic Crystals* (Academic, 2003).

**15. **N. Bloembergen and A. J. Sieveres, “Nonlinear Optical Properties of Periodic Laminar Structures,” Appl. Phys. Lett. **17**(11), 483–486 (1970). [CrossRef]

**16. **C. L. Tang and P. P. Bey, “Phase Matching in Second-Harmonic Generation Using Artificial Periodic Structures,” IEEE J. Quantum Electron. **9**(1), 9–17 (1973). [CrossRef]

**17. **J. P. van der Ziel and M. Ilegems, “Optical second harmonic generation in periodic multilayer GaAs-Al_{0.3}Ga_{0.7}As structures,” Appl. Phys. Lett. **28**(8), 437–439 (1976). [CrossRef]

**18. **C. M. Bowden and A. M. Zheltikov, “Nonlinear Optics of Photonic Crystals,” J. Opt. Soc. Am. B **19**(9), 2046–2048 (2002). [CrossRef]

**19. **E. Centeno, “Second-harmonic superprism effect in photonic crystals,” Opt. Lett. **30**(9), 1054–1056 (2005). [CrossRef]

**20. **K. S. Novoselov, A. K. Geim, S. V. Morozov, D. Jiang, M. I. Katsnelson, I. V. Grigorieva, S. V. Dubonos, and A. A. Firsov, “Two-dimensional gas of massless Dirac fermions in graphene,” Nature **438**(7065), 197–200 (2005). [CrossRef]

**21. **A. H. Neto, F. Guinea, N. M. R. Peres, K. S. Novoselov, and A. K. Geim, “The electronic properties of graphene,” Rev. Mod. Phys. **81**(1), 109–162 (2009). [CrossRef]

**22. **F. D. M. Haldane and S. Raghu, “Possible Realization of Directional Optical Waveguides in Photonic Crystals with Broken Time-Reversal Symmetry,” Phys. Rev. Lett. **100**(1), 013904 (2008). [CrossRef]

**23. **S. Raghu and F. D. M. Haldane, “Analogs of quantum-Hall-effect edge states in photonic crystals,” Phys. Rev. A **78**(3), 033834 (2008). [CrossRef]

**24. **R. A. Sepkhanov, Ya. B. Bazaliy, and C. W. J. Beenakker, “Extremal transmission at the Dirac point of a photonic band structure,” Phys. Rev. A **75**(6), 063813 (2007). [CrossRef]

**25. **X. Zhang, “Observing *Zitterbewegung* for Photons near the Dirac Point of a Two-Dimensional Photonic Crystal,” Phys. Rev. Lett. **100**(11), 113903 (2008). [CrossRef]

**26. **M. Diem, T. Koschny, and C. M. Soukoulis, “Transmission in the vicinity of the Dirac point in hexagonal photonic crystals,” Physica B **405**(14), 2990–2995 (2010). [CrossRef]

**27. **X. Huang, Y. Lai, Z. H. Hang, H. Zheng, and C. T. Chan, “Dirac cones induced by accidental degeneracy in photonic crystals and zero-refractive-index materials,” Nat. Mater. **10**(8), 582–586 (2011). [CrossRef]

**28. **K. Sakoda, “Double Dirac cones in triangular-lattice metamaterials,” Opt. Express **20**(9), 9925–9939 (2012). [CrossRef]

**29. **G. D’Aguanno, N. Mattiucci, C. Conti, and M. J. Bloemer, “Field localization and enhancement near the Dirac point of a finite defectless photonic crystal,” Phys. Rev. B **87**(8), 085135 (2013). [CrossRef]

**30. **N. Mattiucci, M. J. Bloemer, and G. D’Aguanno, “All-optical bistability and switching near the Dirac point of a 2-D photonic crystal,” Opt. Express **21**(10), 11862–11868 (2013). [CrossRef]

**31. ***Handbook of Optical Constants of Solids*, E. D. Palik ed. (Academic Inc., 1991).

**32. **L. Li, “Formulation and comparison of two recursive matrix algorithms for modeling layered diffraction gratings,” J. Opt. Soc. Am. A **13**(5), 1024–1035 (1996). [CrossRef]

**33. **B. Gralak, S. Enoch, and G. Tayeb, “Anomalous refractive properties of photonic crystals,” J. Opt. Soc. Am. A **17**(6), 1012–1020 (2000). [CrossRef]

**34. **G. D’Aguanno, M. Centini, M. Scalora, C. Sibilia, M. Bertolotti, M. J. Bloemer, and C. M. Bowden, “Generalized coupled-mode theory for χ^{(2)} interactions in finite multilayered structures,” J. Opt. Soc. Am. B **19**(9), 2111–2121 (2002). [CrossRef]

**35. **N. Mattiucci, G. D’Aguanno, M. Scalora, and M. J. Bloemer, “Coherence Length during a SH Generation Process in Nonlinear, One-Dimensional, Finite, Multilayered Structures,” J. Opt. Soc. Am. B **24**, 877–886 (2007). [CrossRef]