Asymmetric nonlinear-mode-conversion in an optical waveguide withPT symmetry

Changdong Chen, Youwen Liu, Lina Zhao, Xiaopeng Hu, Yangyang Fu

Front. Phys. ›› 2022, Vol. 17 ›› Issue (5) : 52504.

PDF(4809 KB)
Front. Phys. All Journals
PDF(4809 KB)
Front. Phys. ›› 2022, Vol. 17 ›› Issue (5) : 52504. DOI: 10.1007/s11467-022-1177-y
RESEARCH ARTICLE
RESEARCH ARTICLE

Asymmetric nonlinear-mode-conversion in an optical waveguide withPT symmetry

Author information +
History +

Abstract

Asymmetric mode transformation in waveguide is of great significance for on-chip integrated devices with one-way effect, while it is challenging to achieve asymmetric nonlinear-mode-conversion (NMC) due to the limitations imposed by phase-matching. In this work, we theoretically proposed a new scheme for realizing asymmetric NMC by combining frequency-doubling process and periodic PT symmetric modulation in an optical waveguide. By engineering the one-way momentum from PT symmetric modulation, we have demonstrated the unidirectional conversion from pump to second harmonic with desired guided modes. Our findings offer new opportunities for manipulating nonlinear optical fields with PT symmetry, which could further boost more exploration on on-chip nonlinear devices assisted by non-Hermitian optics.

Graphical abstract

Keywords

nonlinear mode conversion / meta-grating / PT symmetry / optical waveguide

Cite this article

Download citation ▾
Changdong Chen, Youwen Liu, Lina Zhao, Xiaopeng Hu, Yangyang Fu. Asymmetric nonlinear-mode-conversion in an optical waveguide withPT symmetry. Front. Phys., 2022, 17(5): 52504 https://doi.org/10.1007/s11467-022-1177-y

1 Introduction

Owing to the abundance of non-conservative processes in optical fields, the concept of parity−time (PT) symmetry, first proposed in quantum mechanics [1, 2], has been introduced into photonics and attracted considerable attentions in recent years [3, 4]. By implementing optical PT symmetry with refractive index profile n(y)=n(y), varieties of intriguing phenomena have been discovered in various optical systems [5-18], such as optical waveguides [5-7], lasers [8-10], optical resonators [11-14], dissimilar antenna-type resonators [15, 16]. The concept of PT symmetry is further developed as non-Hermitian optics [19], in which spatially engineering gain and/or loss are considered to manipulate optical fields. In particular, much attention has been taken in the non-Hermitian modulation with a periodical refractive index Δn=ρ1cos(qy)+iρ2sin(qy), which enables a one-way momentum at the exceptional point with ρ1=ρ2. Utilizing this unique property in active/passive optical systems, many interesting wave phenomena and novel applications [19-31] have been investigated, for instance, non-reciprocal light propagation [20-24], unidirectional invisibility [25-27], asymmetric diffraction [28]. While all these prior arts developed from the one-way momentum are largely locked in linear waves, and it is significant to introduce them into nonlinear optics, which could offer new paradigms to explore new nonlinear effects, such as one-way second harmonic (SH) generation, and mode-convertor.
As known, the key issue of nonlinear interactions within waveguide (e.g., LiNbO3 (LN) waveguide) is the momentum (phase) mismatch, resulting from dispersions both in materials and guided modes. The most common way to solve such a problem is employing poled quasi-phase-matching structures [32, 33], which can compensate for the momentum mismatch between fundamental wave (FW) and SH modes. Although some other ways [34, 35] have been proposed to realize the momentum match in the process of nonlinear interactions, all these structures therein are impossible to realize asymmetric performance for nonlinear-mode-conversion (NMC), i.e., FW to SH. Here we proposed and demonstrated a new way for achieving NMC with asymmetric response in a LN waveguide with PT symmetry. The underlying mechanism lies in that the frequency-doubling process in the waveguide is designed to obtain the higher-mode of SH from the fundamental mode of FW and then unidirectional mode conversion from the higher-mode to the fundamental mode of SH is generated by the one-way momentum from PT symmetry. This work may open up a new way to obtain SH generator and expands the current capabilities of nonlinear devices.

2 The model of asymmetric NMC

Fig.1(a) schematically shows our considered structure, which is comprised of a single z-cut LN film layer and a buried SiO2 layer underneath LN film. Periodically arranged optical potentials Δϵ(y)=cos(qy)+isin(qy), along the light propagation in the y direction, are implemented on the LN waveguide with dielectric constant ϵr. To be exact, the LN waveguide is in possession of a perturbative PT symmetry profile, i.e., ϵ(y)=ϵr+Δϵ(y). Such a periodically active and passive modulations can form a long-period grating with a period of Λ. This type of periodic modulation will possess a y-dependent perturbation function ξ(y)=eiqy where q=2π/Λ, and here we set the origin as the starting point of the initial modulation period. Obviously from its Fourier transform, a unidirectional wave-vector (momentum) q can be introduced along y-direction, which can interact with the guided modes in LN film. Utilizing this feature, it is feasible to obtain unidirectional conversion from FW to SH with desired guided modes by devising specific nonlinear interactions and modulation periods in the waveguide.
Fig.1 (a) The schematic configuration of asymmetric NMC. Active and passive modulations taking a period of Λ, with Δϵ(y)=cos(qy)+isin(qy), are applied on the LN waveguide layer with a thickness of d= 1.01 μm, giving rise to a one-way wave-vector q along y direction. (b) The mode dispersions in LN waveguide for FW (from 0.8 μm to 1.6 μm) and the corresponding SH. There is only one intersection at about 1.064 μm that is a probable FW wavelength to realize phase-matched frequency-doubling process. (c) Forward and backward phase-matching conditions induced by PT symmetry for TM22ω mode in the dispersion diagram of SH. (d) The sketch map of entire process of the asymmetric NMC only for forward-propagation, can two FW photons (0th order mode) be transformed into one SH photon (0th order mode) via the coupling between the interactions resulting from nonlinearity and PT symmetry.

Full size|PPT slide

Besides the one-way wave-vector, another critical issue is to realize pronounced frequency-doubling process for efficient nonlinear mode transformation. We show the mode dispersions of FW (wavelength regime from 0.8 μm to 1.6 μm) and SH (0.4 to 0.8 μm) of the LN waveguide in Fig.1(b), where the waveguide parameters are 1.01 μm and 10 μm respectively for LN film and SiO2 layer. Note that TM (electric field alongz-polarization) waves are just considered here in order to exploit the largest nonlinear coefficient d33 of LN crystal. There is only one intersection point at FW of 1.064 μm (the green point in Fig.1(b)) among distinct dispersion lines. This point is exactly the phase-matching point that allows to achieve considerable TM22ω (2nd order of SH mode). Since the effective refractive index of FW mode remains lower than that of SH mode for the identical order, it is of great difficulty to realize efficient conversion of TM0ωTM02ω directly, either by regulating waveguide parameters [34, 35], or assisted by meta-surface [36]. However in our scenario, if the generated SH wave satisfies β22ω+q=β02ω, where βi2ω(i=0,1,2,) represents the propagation constant of the ith order of SH mode, then the TM22ω mode of forward propagation can be converted into the TM02ω mode (see the right part of Fig.1(c)). While for backward propagation, as shown in the left part of Fig.1(c), β22ω may be transmitted to the spatial frequency of β22ωq, which is in the non-guided region of waveguide in our case. Accordingly, q has no influence on the TM22ω mode of backward propagation.
The overall process of asymmetric NMC could be understood from in Fig.1(d). Owing to phase matching Δβ=0, two FW photons of TM0ω mode are combined to generate directly one SH photon of TM22ω mode, independent of the propagation direction. For the forward process, the SH photon of TM22ω mode will be converted into TM02ω mode via the additional wave-vector q from PT symmetry. While for the backward case, the wave-vector q cannot be involved in the interaction, the phase-matching is unable and then the TM22ω mode of SH photon is unchanged.

3 Results and discussion

To well simulate the whole interactions, an approach analogous to the split-step Fourier method has been employed. In propagating over a small distance, the nonlinear frequency conversion and PT induced mode conversion can be assumed to act independently for the optical field, while they act together along the whole length of waveguide. Consequently, the dynamics of nonlinear interaction can be derived as
dA0ωdy=iωNeff02ωc[κ10A02ω(A0ω)eiΔβ0y+κ12A22ω(A0ω)eiΔβ2y],
dA02ωdy=iωNeff02ωc(κ20(A0ω)2eiΔβ0y),
dA22ωdy=iωNeff22ωc(κ22(A0ω)2eiΔβ2y),
where Anω(2ω) represents the amplitude of the nth order of FW (SH) mode; Neffnω(2ω) represents the effective refractive index of the nth order of FW (SH) mode; ω is the circular frequency of FW; κ10(2)and κ20(2) are nonlinear coupling coefficients and can be expressed as
κ10(2)=(E0ω(z))χ(2):E0(2)2ω(z)(E0ω(z))dzE0ω(z)(E0ω(z))dz,
κ20(2)=(E0(2)2ω(z))χ(2):E0ω(z)E0ω(z)dzE0(2)2ω(z)(E0(2)2ω(z))dz,
in which Enω(2ω) represents the transverse field distribution of the nth order of FW (SH) mode and χ(2) is nonlinear susceptibility tensor; Δβj is the momentum mismatch of the nonlinear interaction between fundamental mode of FW and the jth mode of SH. In addition, as discussed above, mode conversion process induced by PT symmetry should be coupled with these nonlinear interactions simultaneously. Thus, other two dynamic equations should be included:
dA02ωdy=iγ1ξ(y)A02ω(y)+iγ2ξ(y)A22ω(y)eiΔβ3y,
dA22ωdy=iγ3ξ(y)A02ω(y)eiΔβ3y+iγ4ξ(y)A22ω(y),
in which the coupling coefficients are described as follows:
γ1=ω22(β02ω)c2(E02ω(z))ΔξE02ω(z)dz|E02ω(z)|2dz,
γ2=ω22(β02ω)c2(E02ω(z))ΔξE22ω(z)dz|E02ω(z)|2dz,
γ3=ω22(β22ω)c2(E22ω(z))ΔξE02ω(z)dz|E22ω(z)|2dz,
γ4=ω22(β22ω)c2(E22ω(z))ΔξE22ω(z)dz|E22ω(z)|2dz.
Here Δβ3=β02ωβ22ω, and Δξ represents the modulation depth of the perturbation function.
If no PT structure is loaded, i.e. Δξ=0, nonlinear interaction will play a dominant role in the propagation. In general, frequency-doubling efficiency of each SH mode is decided collaboratively by both nonlinear coupling coefficient (overlapping integral of guided modes) and phase-matching condition. Therefore, in our simulations, we consider two cases of nonlinear transfer of TM22ω and TM02ω modes. As depicted in Fig.2, with the depletion of FW, the weak intensity of TM02ω mode oscillates with propagation distance and ultimately tend to a stable value. While for TM22ω mode, its intensity, just as we designed, grows with the increase of length and is about six orders of magnitude higher than that of TM02ω mode. This result also indicates that phase-matching is the key factor, although κ10, κ20 for TM02ω mode are about 23 times and 2 times κ12, κ22 for TM22ω mode based on the calculations in our model respectively. Due to the reciprocity of frequency-doubling, the simulation results are identical, either for forward-propagating or backward-propagating of FW.
Fig.2 The dependences of nonlinear mode conversion on propagation distance without PT-symmetry modulation. (a) TM0ω mode of FW. (b) TM02ω mode of SH. (c) TM22ω mode of SH.

Full size|PPT slide

Subsequently, we consider the situations with PT modulation. Then, for the forward case, Eqs. (6) and (7) are revised as
dA02ωdy=iγ1A02ω(y)eiqy+iγ2A22ω(y)ei(Δβ3q)y,
dA22ωdy=iγ3A02ω(y)ei(q+Δβ3)y+iγ4A22ω(y)eiqy.
In terms of our calculated results of Δβ3, the selected q is set to be 1.4226 μm−1 under which the second exponential term of Eq. (12) will vanish. Meanwhile, these two procedures, nonlinear SH and mode conversion induced by PT, are tightly coupled with each other, and the nonlinear process provides an essential value of A22ω. Consequently, the intensity of TM02ωmode is enhanced as the propagation distance increases, as shown in Fig.3(b). On the other hand, in virtue of the one-way nature of q, both the exponential terms of Eq. (13) cannot be neglected, which limits the chance that the generated TM02ω mode turns back into TM22ω mode. So, the contribution to TM22ω mode intensity mainly comes from nonlinear SH interaction. As demonstrated in Fig.3(a) and (c), the intensity of TM0ω mode is gradually converted into that of TM22ω mode owing to the phase matching between these two modes. Besides, it is seen TM22ω mode power remains oscillation as it grows with the propagation length. This is also caused by the coupling between the aforesaid two primary processes. Hence, when TM22ω mode propagates along the y direction, the phase-mismatch enlarged by q in Eq. (13) will result in such oscillation along with a phase-matched SH process. Moreover, as illustrated in Fig.3(b), this oscillation feature also takes place for TM02ω mode, which is principally determined by two aspects consisting of the oscillating TM22ω mode intensity and the residual exponential term in Eq. (12). To reveal clearly these features, the polynomial fitting curves (green dot lines) have been calculated and displayed in Fig.3.
Fig.3 Asymmetric mode conversion with nonlinearity and PT-symmetry modulation together. The mode intensities, respectively for TM0ω mode of FW, TM02ω mode of SH and TM22ω mode of SH, vary with the change of propagation distance under the situations of forward-propagation (ac) and backward-propagation (df).

Full size|PPT slide

While for the backard case, the dynamics can be derived as
dA02ωdy=iγ1A02ω(y)eiqyiγ2A22ω(y)ei(q+Δβ3)y,
dA22ωdy=iγ3A02ω(y)ei(qΔβ3)yiγ4A22ω(y)eiqy.
In contrast with the forward case, the selected q cannot compensate for the mismatch in Eq. (14), but magnifies it instead. It somewhat restrains TM22ω mode from converting into TM02ω mode. As depicted in Fig.3(e), the intensity of TM02ω mode gradually oscillates to a nearly stable value which is approximately three orders lower than that in the forward case. In addition, one can find the first exponential term of Eq. (15) can be cancelled, indicating that TM02ω mode could be transferred into TM22ω mode. However, in our scheme, the conversion from TM0ω mode to TM02ω mode, as demonstrated in Fig.2(b), is extremely inefficient, which means nonlinear interaction cannot offer sufficient A02ω to support this PT-symmetry induced interaction. Hence for TM22ω mode as shown in Fig.3(f), it is analogous to the forward case that the intensity is decided largely in frequency-doubling process.
The foregoing comparative analysis of Fig.3 demonstrates such a mode conversion in waveguide, with the coupling of nonlinearity and PT symmetry, can be realized and asymmetric. Owing to the involvement of PT symmetry, this type of mode conversion correlates strongly with the modulation depth Δξ. As illustrated in Eqs. (6) and (7), the coupling coefficients γi that are attributable to PT symmetry are proportional to Δξ. For the forward propagation, the output intensity of TM02ω mode mainly relies on the coefficient γ2. As shown in Fig.4, it is found that a greater modulation depth will achieve a higher value of γ2, and consequently leads to a larger transformed mode intensity that grows exponentially with Δξ. Besides, the other three coefficients γ1, γ3 and γ4 determine the oscillation property of output modes. From the insets of Fig.4, respectively for Δξ=0,Δξ=0.25 and Δξ=0.45, we can clearly see that the amplitude of oscillation rises with the increase of Δξ.
Fig.4 The excited TM02ω mode intensity changes with the variation of the modulation depth of PT-symmetry. The insets illustrate the mode intensities that can be eventually generated with distinct modulation depth Δξ=0, Δξ=0.25 and Δξ=0.45.

Full size|PPT slide

For the above theoretical analysis, we employ an ideal model of PT symmetry with balanced gain and loss for a one-way wave-vector to demonstrate the asymmetric NMC, while similar results could be realized by considering other simple ways, such as passive PT systems [19, 24]. In terms of our simulations where a purely passive system is taken, the performance of NMC is demonstrated in Fig.5. Compared with the ideal case, the efficiency of NMC shown in Fig.5(a) becomes lower. On the other hand, despite no linear gain, nonlinear SH process provides an initial stimulation of the cascaded mode conversion induced by PT, when the pump propagates over each short distance in the waveguide. Meanwhile, the efficiency of this nonlinear process is proportional to the square of propagation length, which implies that the stimulation to NMC will enhance along the propagation direction of FW. Consequently, the efficiency of NMC can continue to grow provided that the nonlinear process is not particularly inefficient. This feature is significantly distinct from that in the case of a single linear passive system without nonlinearity. In that case, the stimulation to mode conversion gradually diminishes with the growing distance, which will make the conversion efficiency increase first and then decrease. Obviously, the reason leading to this difference in efficiency, in contrast with our NMC scheme, lies in the coupling between the nonlinear and linear interactions.
Fig.5 Asymmetric NMC in a purely passive system respectively for the forward (a, b) and backward (c, d) propagations.

Full size|PPT slide

At this point, we have primarily concerned with the NMC in an identical direction, i.e., the converted SH propagates along the input direction of FW. However, utilizing our scheme, can “reflected” NMC be implemented? For instance, the system is excited by a negative-y-propagating FW mode (the backward case in Fig.1(a)), generating a positive-y-propagating (“reflected”) SH mode. In traditional nonlinear optics, such a counter propagating coupling, in general, is tough to be achieved, since the “reflected” SH and the FW modes cannot fulfill the conservation of momentum. To overcome this issue, the most direct way is to address nonlinear process itself, such as employing negative-index [37] or zero-index [38, 39] metamaterials. Unlike this kind of thought, we can transfer the momentum (phase) mismatch from nonlinear process to linear process, owing to the coupling between the nonlinear and linear interactions assisted by PT symmetric modulation. Therefore, in our case, the negative-y-propagating FW mode will still effectively generate negative-y-propagating SH mode TM22ω with a propagation constant β22ω, which is dominated by the mode dispersion in Fig.1(b). And then, this negative-y-propagating SH mode is subsequently converted into the “reflected” SH mode TM22ω with a propagation constant β22ω, provided that β22ωq=β22ω. This relationship is different from that in the case of Fig.3 or Fig.5 where q is so small that β22ωq is located in the non-guided region of Fig.1(c). Therefore, we only require a lager q=2β22ω that can make β22ω “flip” over the non-guided region to the positive-y region, and thus realize “reflected” NMC. Under this circumstance, if the system is excited by a positive-y-propagating FW mode (the forward case in Fig.1(a)), the phase mismatch for the counter propagating coupling still exists so that “reflected” NMC cannot take place. Consequently, it is analogous to the case in Fig.3 that such type of “reflected” NMC remains asymmetric.

4 Conclusion

In conclusion, we have demonstrated the asymmetric NMC by combining frequency-doubling process and periodic PT symmetric modulation in a planar LN waveguide. Following the basic principle, asymmetric generation of SH modes from FW could be arbitrarily designed. For example, this scheme of asymmetric NMC can be potentially applied in a multi-channel configuration, in which each channel is engineered with a reasonable modulation period, and then asymmetric switchover between several desired SH modes on a single chip could be manipulated in a diverse way. Note that we only consider TM mode conversion coupled with nonlinear interaction type of TM+TMTM for above discussion. Actually, there are other three interaction options in general: TM+TMTE, TE+TETE and TE+TETM, and effective asymmetric NMC is greatly dependent on the efficiency of nonlinear process. However, the nonlinear coupling coefficients or dominated nonlinear coefficients (d22 and d31) in these three cases are pretty small, so as to result in inefficient nonlinear mode couplings and interactions. Meanwhile, the frequency-doubling process here could be extended to other nonlinear interactions, including sum-frequency generation, third harmonic generation and four-wave mixing. Our proposed way, therefore, could be further developed to manipulate nonlinear fields with asymmetric response, which can provide a feasible avenue toward designing new nonlinear devices enabled by non-Hermitian optics and meta-optics.

References

[1]
C. M. Bender , S. Boettcher . Real spectra in Non-Hermitian Hamiltonians Having PT symmetry. Phys. Rev. Lett., 1998, 80( 24): 5243
CrossRef ADS Google scholar
[2]
G. Y. Sun , J. C. Tang , S. P. Kou . Biorthogonal quantum criticality in non-Hermitian many-body systems. Front. Phys., 2022, 17( 3): 33502
CrossRef ADS Google scholar
[3]
R. El-Ganainy , K. G. Makris , M. Khajavikhan , Z. H. Musslimani , S. Rotter , D. N. Christodoulides . Non-Hermitian physics and PT symmetry. Nat. Phys., 2018, 14( 1): 11
CrossRef ADS Google scholar
[4]
M. A. Miri , A. Alu . Exceptional points in optics and photonics. Science, 2019, 363( 6422): eaar7709
CrossRef ADS Google scholar
[5]
A. Guo , G. J. Salamo , D. Duchesne , R. Morandotti , M. Volatier-Ravat , V. Aimez , G. A. Siviloglou , D. N. Christodoulides . Observation of PT-symmetry breaking in complex optical potentials. Phys. Rev. Lett., 2009, 103( 9): 093902
CrossRef ADS Google scholar
[6]
Y. Fu , Y. Xu , H. Chen . Zero index metamaterials with PT symmetry in a waveguide system. Opt. Express, 2016, 24( 2): 1648
CrossRef ADS Google scholar
[7]
A. Laha , S. Dey , H. K. Gandhi , A. Biswas , S. Ghosh . Exceptional point and toward mode-selective optical isolation. ACS Photonics, 2020, 7( 4): 967
CrossRef ADS Google scholar
[8]
H. Hodaei , M. A. Miri , M. Heinrich , D. N. Christodoulides , M. Khajavikhan . Parity−time-symmetric microring lasers. Science, 2014, 346( 6212): 975
CrossRef ADS Google scholar
[9]
B. Peng , S. K. Ozdemir , M. Liertzer , W. J. Chen , J. Kramer , H. Yilmaz , J. Wiersig , S. Rotter , L. Yang . Chiral modes and directional lasing at exceptional points. Proc. Natl. Acad. Sci. USA, 2016, 113( 25): 6845
CrossRef ADS Google scholar
[10]
N. Zhang , Z. Y. Gu , K. Y. Wang , M. Li , L. Ge , S. M. Xiao , Q. H. Song . Quasiparity−time symmetric microdisk laser. Laser Photonics Rev., 2017, 11( 5): 1700052
CrossRef ADS Google scholar
[11]
L. Chang , X. S. Jiang , S. Y. Hua , C. Yang , J. M. Wen , L. Jiang , G. Y. Li , G. Z. Wang , M. Xiao . Parity–time symmetry and variable optical isolation in active–passive-coupled microresonators. Nat. Photonics, 2014, 8( 7): 524
CrossRef ADS Google scholar
[12]
B. Peng , S. K. Ozdemir , F. C. Lei , F. Monifi , M. Gianfreda , G. L. Long , S. H. Fan , F. Nori , C. M. Bender , L. Yang . Parity–time-symmetric whispering-gallery microcavities. Nat. Phys., 2014, 10( 5): 394
CrossRef ADS Google scholar
[13]
C. D. Chen , L. N. Zhao . The effect of thermal-induced noise on doubly-coupled-ring optical gyroscope sensor around exceptional point. Opt. Commun., 2020, 474 : 126108
CrossRef ADS Google scholar
[14]
C. D. Chen , Y. J. Xie , S. W. Huang . Nanophotonic optical gyroscope with sensitivity enhancement around “mirrored” exceptional points. Opt. Commun., 2021, 483 : 126674
CrossRef ADS Google scholar
[15]
M. Chen , Z. F. Li , X. Tong , X. D. Wang , F. H. Yang . Manipulating the critical gain level of spectral singularity in active hybridized metamaterials. Opt. Express, 2020, 28( 12): 17966
CrossRef ADS Google scholar
[16]
Y. Liang , Q. Gaimard , V. Klimov , A. Uskov , H. Benisty , A. Ramdane , A. Lupu . Coupling of nanoantennas in loss-gain environment for application in active tunable metasurfaces. Phys. Rev. B, 2021, 103( 4): 045419
CrossRef ADS Google scholar
[17]
Y. Cao , Y. Fu , Q. Zhou , Y. Xu , L. Gao , H. Chen . Giant Goos−Hänchen shift induced by bounded states in opticalPT-symmetric bilayer structures. Opt. Express, 2019, 27( 6): 7857
CrossRef ADS Google scholar
[18]
Y. Fu , Y. Fei , D. Dong , Y. Liu . Photonic spin Hall effect in PT symmetric metamaterials. Front. Phys., 2019, 14( 6): 62601
CrossRef ADS Google scholar
[19]
L. Feng , R. El-Ganainy , L. Ge . Non-Hermitian photonics based on parity–time symmetry. Nat. Photonics, 2017, 11( 12): 752
CrossRef ADS Google scholar
[20]
M. Greenberg , M. Orenstein . Irreversible coupling by use of dissipative optics. Opt. Lett., 2004, 29( 5): 451
CrossRef ADS Google scholar
[21]
L. Feng , M. Ayache , J. Q. Huang , Y. L. Xu , M. H. Lu , Y. F. Chen , Y. Fainman , A. Scherer . Nonreciprocal light propagation in a silicon photonic circuit. Science, 2011, 333( 6043): 729
CrossRef ADS Google scholar
[22]
S. N. Ghosh , Y. D. Chong . Exceptional points and asymmetric mode conversion in quasi-guided dual-mode optical waveguides. Sci. Rep., 2016, 6( 1): 19837
CrossRef ADS Google scholar
[23]
D. Chatzidimitriou , A. Pitilakis , T. Yioultsis , E. E. Kriezis . Breaking reciprocity in a non-Hermitian photonic coupler with saturable absorption. Phys. Rev. A, 2021, 103( 5): 053503
CrossRef ADS Google scholar
[24]
A. Pitilakis , D. Chatzidimitriou , T. V. Yioultsis , E. E. Kriezis . Asymmetric Si-slot coupler with nonreciprocal response based on graphene saturable absorption. IEEE J. Quantum Electron., 2021, 57( 3): 8400210
CrossRef ADS Google scholar
[25]
Z. Lin , H. Ramezani , T. Eichelkraut , T. Kottos , H. Cao , D. N. Christodoulides . Unidirectional invisibility induced by PT-symmetric periodic structures. Phys. Rev. Lett., 2011, 106( 21): 213901
CrossRef ADS Google scholar
[26]
L. Feng , Y. L. Xu , W. S. Fegadolli , M. H. Lu , J. E. B. Oliveira , V. R. Almeida , Y. F. Chen , A. Scherer . Experimental demonstration of a unidirectional reflectionless parity−time metamaterial at optical frequencies. Nat. Mater., 2013, 12( 2): 108
CrossRef ADS Google scholar
[27]
Y. F. Jia , Y. X. Yan , S. V. Kesava , E. D. Gomez , N. C. Giebink . Passive parity−time symmetry in organic thin film waveguides. ACS Photonics, 2015, 2( 2): 319
CrossRef ADS Google scholar
[28]
X. Y. Zhu , Y. L. Xu , Y. Zou , X. C. Sun , C. He , M. H. Lu , X. P. Liu , Y. F. Chen . Asymmetric diffraction based on a passive parity−time grating. Appl. Phys. Lett., 2016, 109( 11): 111101
CrossRef ADS Google scholar
[29]
H. Zhao , W. S. Fegadolli , J. K. Yu , Z. F. Zhang , L. Ge , A. Scherer , L. Feng . Metawaveguide for asymmetric interferometric light−light switching. Phys. Rev. Lett., 2016, 117( 19): 193901
CrossRef ADS Google scholar
[30]
W. Wang , L. Q. Wang , R. D. Xue , H. L. Chen , R. P. Guo , Y. M. Liu , J. Chen . Unidirectional excitation of radiative-loss-free surface plasmon polaritons in PT-symmetric systems. Phys. Rev. Lett., 2017, 119( 7): 077401
CrossRef ADS Google scholar
[31]
Y. Y. Fu , Y. D. Xu , H. Y. Chen . Negative refraction based on purely imaginary metamaterials. Front. Phys., 2018, 13( 4): 134206
CrossRef ADS Google scholar
[32]
L. Chang , Y. F. Li , N. Volet , L. Wang , J. Peters , J. E. Bowers . Thin film wavelength converters for photonic integrated circuits. Optica, 2016, 3( 5): 531
CrossRef ADS Google scholar
[33]
M. Jankowski , C. Langrock , B. Desiatov , A. Marandi , C. Wang , M. Zhang , C. R. Phillips , M. Loncar , M. M. Fejer . Ultrabroadband nonlinear optics in nanophotonic periodically poled lithium niobate waveguides. Optica, 2020, 7( 1): 40
CrossRef ADS Google scholar
[34]
D. H. Sun , Y. W. Zhang , D. Z. Wang , W. Song , X. Y. Liu , J. B. Pang , D. Q. Geng , Y. H. Sang , H. Liu . Microstructure and domain engineering of lithium niobate crystal films for integrated photonic applications. Light Sci. Appl., 2020, 9( 1): 197
CrossRef ADS Google scholar
[35]
R. Luo , Y. He , H. X. Liang , M. X. Li , Q. Lin . Highly tunable efficient second-harmonic generation in a lithium niobate nanophotonic waveguide. Optica, 2018, 5( 8): 1006
CrossRef ADS Google scholar
[36]
C. Wang , Z. Y. Li , M. H. Kim , X. Xiong , X. F. Ren , G. C. Guo , N. F. Yu , M. Loncar . Metasurface-assisted phase-matching-free second harmonic generation in lithium niobate waveguides. Nat. Commun., 2017, 8( 1): 2098
CrossRef ADS Google scholar
[37]
A. Rose , D. Huang , D. R. Smith . Controlling the second harmonic in a phase-matched negative-index metamaterial. Phys. Rev. Lett., 2011, 107( 6): 063902
CrossRef ADS Google scholar
[38]
A. Rose , D. R. Smith . Overcoming phase mismatch in nonlinear metamaterials. Opt. Mater. Express, 2011, 1( 7): 1232
CrossRef ADS Google scholar
[39]
H. Suchowski , K. O’Brien , Z. J. Wong , A. Salandrino , X. Yin , X. Zhang . Phase mismatch–free nonlinear propagation in optical zero-index materials. Science, 2013, 342( 6163): 1223
CrossRef ADS Google scholar

Acknowledgements

This work was supported by the National Natural Science Foundation of China (Grant Nos. 11904169 and 91950106), the Fundamental Research Funds for the Central Universities (Grant No. NE2022007), the Natural Science Foundation of Jiangsu Province (No. BK20190383), Postdoctoral Science Foundation of Jiangsu Province (No. 2020Z224), China Postdoctoral Science Foundation (No. 2020M681576), and the Top-notch Academic Programs Project of Jiangsu Higher Education Institutions.

Disclosures

The authors declare no conflicts of interest.

Data availability

Data underlying the results presented in this paper are not publicly available at this time but may be obtained from the authors upon reasonable request.

RIGHTS & PERMISSIONS

2022 Higher Education Press
AI Summary AI Mindmap
PDF(4809 KB)

743

Accesses

7

Citations

Detail

Sections
Recommended

/