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Selfinduced transparency in a perfectly absorbing chiral secondharmonic generator
PhotoniX volume 3, Article number: 22 (2022)
Abstract
Transparency and perfect absorption are two contradictory terms; a perfect absorber never permits waves to transmit through. However, this statement only remains true in the linear regime, where the nonlinearity has been omitted and the physical system like the perfect absorber is not affected by the incoming waves. Here we experimentally demonstrate an intriguing selfinduced transparency effect in a perfectly absorbing optical microcavity, which perfectly absorbs any incoming waves at the low power level, but allows a portion of waves to be transmitted at the higher power due to the nonlinear coupling between the fundamental and its second harmonic modes. Moreover, the asymmetric scattering nature of the microcavity enables a chiral and unidirectional reflection in one of the input ports, this leads to asymmetric and chiral coherent control of the perfect absorption states through phase varying. More importantly, such chiral behaviors also empower the chiral emission of secondharmonic generation with a high distinct ratio in the transparency state. These results pave the way for controllable transparency in a wide range of fields in optics, microwaves, acoustics, mechanics, and matter waves.
Introduction
Perfect absorption of the incoming radiation is crucial for many interdisciplinary areas in optics [1, 2], microwaves [3], acoustics[4], mechanics[5], as well as matter waves[6]. One representative example, namely, coherent perfect absorber (CPA) delicately constructs lossy geometry into a cavity design by considering an exact timereversed laser. This leads to a spectral “blackhole” singularity, a mathematical notion where the system perfectly absorbs any incoming wave without reemitting [1]. Although firstly proposed and implemented in optics, CPA quickly spans all areas of classical wave systems from microwave to acoustics[1,2,3,4,5,6]. More importantly, CPA promises a wide range of practical applications in optical information processing[7], energy harvesting[8], photodetection[9], and sensing[10].
Transparency and perfect absorption seem to be a paradox at the first glance, a perfect absorber never permits waves to transmit through. However, this is mainly because most of the prior works are implemented in the linear regime, i.e. incoming waves do not affect the perfect absorber itself. Contrarily, waves’ amplitude can greatly alter the dynamics of absorption in the nonlinear regime, which is more universal and common in real physical systems. A nonlinear version of CPA has been theoretically studied [11], but only limited to their nonlinear dynamics. Such devices are usually composed of a sandwich structure with an embedded nonlinear absorbing layer, which creates an extra obstacle to meet the CPA condition. For example, nonlinearity leads to a selfinduced perfect absorption above a certain critical value with microwave [12]; And the CPA of nonlinear matter waves in an atomic BoseEinstein condensate can be achieved easier than its linear analogs because of the strength of twobody interaction nonlinearity [6]. Hence, transparency can be much anticipated, though no experimental observation yet, in a nonlinear version of CPA.
On the other hand, transparency indeed can be achieved through an externally controlled manner in an opaque /absorbing medium. In atomic physics, electromagnetically induced transparency (EIT) allows the flipping of an optical opaque window to a transparent one under a secondary coherent illumination beam even at the fewphoton limit[13]. This process provides tremendous opportunities for quantum physics and information science, enabling applications in alloptical and quantum information processing, slow/fast light, and photon storage[13,14,15,16]. Later, by recognizing the interference effect as the key working mechanism behind EIT, classical analogies that mimic the EIT effect are under active pursuit in various physical systems, including microresonators[7, 17,18,19], photonic crystals[20], and plasmonic metamaterials[21]. However, these works still rely on the externalcontrol mean such as a second laser. Meanwhile, selfinduced transparency has been extensively studied mainly in atomic systems, thanks to the strong nonlinearity of atoms [22, 23], but the associated cooling and vacuum systems halt their practical applications. So far, selfinduced transparency in a perfect absorbing optical cavity has never been reported till this work.
In this work, we experimentally demonstrate a selfinduced transparency effect in a perfectly absorbing optical microcavity, which only totally absorbs lowpower incoming waves in the linear regime, but dramatically turns into a partial transparency state after ramping up the input power. Such selfinduced transparency is introduced by the nonlinear coupling between the optical modes at the fundamental frequency and its second harmonic, causing partially breaking the balance condition of a coherent destructive interference which holds the key to enabling perfect absorption or critical coupling initially in the microcavity. Furthermore, we find the current microcavity device contains a unique asymmetric scattering feature of chiral and unidirectional reflection, which is caused by multiple surface scatters that break the chiral symmetry. As a result, asymmetric and chiral coherent control of the perfect absorption states is realized through phase varying. This coherent control can be further extended into the second harmonic spectrum, resulting in a chiral emission of secondharmonic generation with a high distinct ratio in the transparency state. These results should be general and universal among other physical systems with nonlinearity like microwaves, acoustics, mechanics, and matter waves, hence it paves the way for practical applications in alloptical signal processing and quantum information.
Results and discussion
The original CPA idea composes of two ports geometry to enable perfect absorption in the embedded layer by coherent destructive interference[2]. Oneport CPA can also be realized in a waveguide coupled microcavity scheme (Fig. 1a), in which similar destructive interference between the cavity’s outcoupling light & the residual transmission, also known as critical coupling[24]. This leads to complete and perfect absorption of input waves inside the microcavity, where light energy dissipates in the form of material absorption and surface scattering, while the incoupling portion from the waveguide is exactly balanced by the outcoupling port from the cavity. At this equilibrium state, any perturbation breaking this balance can lead to the disappearance of a perfect absorption state. In the linear regime (Fig. 1b), the incoming waves can hardly disturb the system at low power, in contrast, highpower inputs can trigger the nonlinear response of the system such that the dedicated balance of input and output will be destroyed, resulting in selfinduced transparency in the transmission spectrum (Fig. 1c).
One representative example of such is a microcavity of quadratic secondorder nonlinearity, which allows the second harmonic generation (SHG) from the fundamental wave (FW) frequency \(\omega\) of the incoming waves to its second harmonic \(2\omega\). With a higher input power, a portion of input optical energy is converted into its second harmonic, effectively creating a “nonlinear loss” at the fundamental frequency. As a result, the aforementioned most important balance will be broken, destructing the perfect absorption at \(\omega\) (Fig. 1c). More specifically, we consider a tapered fiber coupled microcavity with secondorder nonlinear susceptibility \({\chi }^{\left(2\right)}\) and internal coupling between clockwise (CW) and counterclockwise (CCW) directions (Fig. 1d), and the evolution dynamics can be described by four sets of coupled rate equations, each at \(\omega\) and \(2\omega\), and in both CW/CCW directions. The governing Hamiltonian is given by \(i\frac{d\psi }{dt}=H\psi\), where \(\psi ={({\alpha }_{1},{\alpha }_{2},{\beta }_{1},{\beta }_{2})}^{T}\)represents field vectors, and \({\alpha }_{1},{\alpha }_{2},{\beta }_{1},{\beta }_{2}\) are the internal cavity amplitudes for CW, CCW waves at \(\omega\), CW, CCW waves at \(2\omega\), respectively. \(H\) is a 4 × 4 nonHermitian Hamiltonian:
where the resonant frequency detuning terms are \({\varDelta }_{1}=(\omega {\omega }_{1})\) at the fundamental frequency, \({\varDelta }_{2}=(2\omega {\omega }_{2})\) at its second harmonic; for each frequency, \({\gamma }_{10}=\left({{\gamma }_{1}+\gamma }_{c1}\right)/2\), \({\gamma }_{20}=\left({{\gamma }_{2}+\gamma }_{c2}\right)/2\) are the effective loss, and \({\gamma }_{c1}\), \({\gamma }_{c2}\) represent the coupling strength with which the cavity coupled to the waveguide; \({\gamma }_{1}\), \({\gamma }_{2}\) are the intrinsic loss terms which are dominated by material absorption and surface impurities; \(g\) is the secondorder nonlinear coupling strength constant determined by \({\chi }^{\left(2\right)}\). The coupling terms \({J}_{12}/{J}_{21}\) and \({I}_{12}/{I}_{21}\) between CW/CCW modes at \(\omega\) and \(2\omega\), respectively, arising from linear scattering. Note that, \(H\) is a nonlinear Hamiltonian as well, whose offdiagonal terms, e.g. \(2{g}^{*}{\alpha }_{1}^{*}\), \(2{g}^{*}{\alpha }_{2}^{*}\), depending on the internal fields \({\alpha }_{1},{\alpha }_{2}\). This is the origin of selfinduced transparency.
For a unidirectional input, i.e. \({\alpha }_{2}=0\), we can simplify \(H\) into a 2 × 2 matrix in supplement S1. Under the steadystate assumption, we can solve the associated coupled rate equations and obtain the transmission rate:
and the intracavity second harmonic amplitude is given by:
In the linear case, i.e. \({\alpha }_{1}\to 0\), Eq. 2 perfectly represents a scenario for singleport CPA, where the critical coupling occurs at \({\gamma }_{c1}={\gamma }_{c}\)[24]. The corresponding transmission spectra exhibit a perfect absorbing dip, i.e. \(T=0\) at the zero detuning point \({\varDelta }_{1}=0\) in Fig. 1b. Nonlinearly, when increasing the signal amplitude \({\alpha }_{1}\), the CPA dip will diminish, allowing a portion of the light to be transmitted, termed as selfinduced transparency (Fig. 1c). Note that, only the income wave signal amplitude has been increased during this process, it is a selfinduced action of signal amplitude in contrast to the linear case at a lower amplitude level. In the meantime, the microcavity starts to generate the second harmonics of the fundamental waves given by Eq. 3, effectively becoming a secondharmonic generator. Moreover, such SHG is resonantly enhanced due to the resonances of the microcavity (Fig. 1c).
In our experiment, a microcavity (Qfactor ~ 10^{6}) with secondorder nonlinearity is fabricated on a lithium niobate on insulator (LNOI) platform [Details in the method section, 25]. As shown in Fig. 1a, the microcavity with a diameter ~ 100\(\mu m\) is coupled with a tapered fiber within which a laser source around the 1550 nm telecommunication band propagates. The laser signals can be launched into both ports of the fiber, which also serve as the output ports for monitoring both the linear transmission and the SHG output on both ports. By slowing scanning the tunable laser at a speed of 0.01 nm/s through the resonances from the reddetuned region, transmission spectra can be obtained in Fig. 2. The tapered fiber is precisely positioned on a piezoelectric stage to tune the gap (~ 100 nm) from the cavity with ~ 10 nanometers resolution, such that careful positioning of the tapered fiber can reach the critical coupling condition in Fig. 2a. Note that, due to the surface scattering from dust, scatter or surface roughness, the CW resonances can be effectively coupled with its counterpart, i.e. counterclockwise (CCW) modes, both at \(\omega\) and \(2\omega\) as shown in Fig. 1d. This coupling mechanism dramatically complicates the dynamics both in the linear regime and nonlinear one, enabling some intriguing effects like unidirectional reflection and chiral SHG, we shall soon discuss them in the following section.
Under this oneport excitation scheme, we experimentally observe a perfect absorption dip with ~ 99% efficiency in the transmission spectrum at the critical coupling condition as shown in Fig. 2a. The incident power of the laser is measured to be ~ 175µW, no SHG is visible at such low power. As the pump laser’s power is gradually tuned up, starting around several milliwatts, a clear SHG signal is detected in the throughport, indicating the energy flow from the fundamental modes to its second harmonics. As a result, the absorption dip begins to reduce in the transmission spectrum. Figure 2b shows such transmission can raise up from almost none to ~ 40% when the pump laser reaches 25.2mW, a sharp contrast to its behavior in the linear regime at low power. This nonlinear dynamic marks selfinduced transparency in the oneport CPA configuration, only depending on the input laser’s power. In the meantime, the SHG signal is also increasing quadratically in Fig. 2c according to the theory in Eq. 3. Moreover, the onresonance transmission T will grow slowly at high pump power and approach 1 when the input power is infinity, which can be easily deduced from Eq. 2. Note that, the original Lorentz lineshape in the linear case is greatly distorted into a triangled one due to the thermalpulling effect [26], but this behavior only shifts the resonances horizontally along the frequency axis, not their transmission [see supplementary S7].
Traditional CPAs are featured with a twoport apparatus for active phase control of the perfect absorption state[2], where coherent control of the relative phases between the two input ports can actively switch between the CPA and the maximum scattering state, or even lasing mode[27]. Given the tapered fiber coupling scheme, it is also possible for us to launch two beams simultaneously from both ports into the microcavity, in which the surface scatters can couple the waves in both directions together, represented in the offdiagonal terms in Eq. 1, e.g. \({J}_{12}\), \({J}_{21}\). In Fig. 3, near a critical coupling condition from a left excitation (Fig. 3a), a nearzero transmitted dip is observed in the transmission, this is companied by a strong reflection to the left, indicating a big scattering factor from CW to CCW mode, i.e. \({J}_{21}\). In a contrast to the right excitation case, a transmission dip with a similar efficiency of ~ 95% is observed, but with a much lower backscattered light to the right port. The similarity between the two transmission spectra is guaranteed by the optical reciprocity [28], while the unequal backscattering arises from the asymmetric scatter distribution inside the cavity. For example, in the inset of Fig. 3a, we do observe two strong outplane scattering signals from the right corner of the microcavity.
Such chiral behaviors, i.e. CPA from both directions and unidirectional reflector, originate from the important fact that the backscattering between intracavity CW and CCW traveling waves is asymmetric, i.e. \({J}_{12}\ne {J}_{21}\)[29, 30], which introduces asymmetric reflection output from the scattering matrix (Smatrix) [31]. Intuitively, this process could be understood as a linear interference between two scattering waves from two scatters at the coupling point, the two scatters have to be distinct in terms of their scattering coefficients to break the chirality [29]. Previously, this very idea has been testified to realize chiral modes and directional lasing at exceptional points in a microcavity[32]; More recently, CPA on an exceptional surface with a chiral reflection has also been demonstrated with a mirror coupled microcavity device[33]. Our fabricated microcavity naturally contains such asymmetrical surface scattering properties due to fabrication defects or external dust as shown in Fig. 3a, it enables us to observe for the first time, to our knowledge, such chiral behaviors of CPA in a single microcavity.
This chiral behavior of the oneport CPA has its consequences in its twoport version, especially in the coherent control of the CPA. In the classical twoport CPA experiment, the symmetric lossy cavity ensures the total destructive interferences between the transmitted and reflected beams, simultaneously on both the incident ports. This leads to the perfect absorption only inside the lossy layer[2]. This requires a pair of symmetric equalamplitude incident waves from both sides. However, when such symmetry is broken, for example, with a paritytime symmetric cavity[27], the required ratio between the two ports is not unit anymore. To demonstrate the coherent control of twoport CPA, we launch two beams with unequal power from both ports into the microcavity at the aforementioned critical coupling condition (Fig. 4a). As usual, both transmission spectra under singleport excitation exhibit well complete absorption dips in Fig. 4b, while their corresponding reflection spectra differ by 20dB. In Fig. 4b, by comparing the output spectra from Port 1 (reflection of \({\alpha }_{in1}\) and transmission of \({\alpha }_{in2}\) ) and Port 2 (reflection of \({\alpha }_{in2}\) and transmission of \({\alpha }_{in1}\) ), we can find an optimal spectral point to achieve complete destructive interference when implementing phase control, a similar technique has been used in the original twoport CPA experiment[2].
In the linear regime (low power, no SHG), we observe large power variations from both ports during the phase varying process. Similar to prior works, a complete destructive cancellation of the Port 1’s output is evident in Fig. 4c & g, at which the reflection of \({\alpha }_{in1}\) and the transmission of \({\alpha }_{in2}\) are equal in amplitude (Fig. 4b) and completely out of phase at the \(\pi\) phase difference. As a result, Port 1 can be actively switched on and off purely by phase control. Meanwhile, the output power fluctuation of Port 2 is much milder during the phase varying, simply due to the unequal contributions of the incident waves from both ports. Such chiral behaviors are universal among the other spectral positions, e.g. Figure 4df, where the phase varying does lead to power fluctuations in both ports, but in a synchronous manner. Contrarily, complete destructive cancellations can only be observed in the spectral position depicted in Fig. 4c,g, not others. Particularly, the zerodetuning point, i.e. Figure 4e, is the CPA point in the original symmetric setup in prior work [2], however, this is not the case in the current setup due to the unbalanced reflection and transmission. These experimental observations also match well with the theoretical results calculated using Eq. 1. as shown in Fig. 4cg [supplement S2]. If we increase the input power into the nonlinear regime, the nonlinear loss should be considered, chiral complete absorption will be broken at c&g points[see supplement S4]. Furthermore, we have theoretically proposed a coherent control of such twoport chiral CPAs, which are capable of fully absorbing incident waves from both ports [supplement S3]. But this requires some dedicated design parameters, such as loss factors, not feasible in the current experiments, we will leave it for further investigation.
More interestingly, this chiral dynamic can be translated into a nonlinear regime, a phasecontrollable chiral second harmonic generation can be directly observed as the result of its interference between CW and CCW mode at the FW frequency. It is wellknown that the SHG has to be restricted into a welldefined direction due to the phasematching condition. In the case of the oneport nonlinear CPA shown above, the induced SHG is in the forward direction, the same as its pump beam at the fundamental frequency (Fig. 2). Under the twoport illumination (Fig. 4), the SHG in both CW and CCW directions can intermix directly with each other due to the presentence of surface scattering, i.e. \({I}_{12}/{I}_{21}\) in Eq. 1, or in an indirect manner, the CW/CCW modes of fundamental waves intermix first through \({J}_{12}/{J}_{21}\), then affect their SHGs [see supplementary S4]. Effectively, this also creates a twopath quantum interferences scheme in Fig. 1d, a very important route for coherent quantum control [34]. In the current study, we find the second indirect route domain, especially when the SHG signals are relatively weak with a low conversion efficiency of ~ 0.1%. We still observe the coherent control SHG signals from both output ports due to the phase varying of their fundamental waves in Fig. 5.
Fig. 5ac shows several typical cases of the phasecontrolled SHGs with multiple CW/CCW pump intensity ratios. All the results are measured at the zerodetuning point of the fundamental waves, i.e. \({\varDelta }_{1}=0\), at which the incident beams with various intensity ratios \({P}_{right}/{P}_{left}\) are scanned in their relative phases from \(\pi\) to \(\pi\). Here the input power is kept under 1mW to avoid any thermalinduced waveform distortion. When the \({P}_{right}/{P}_{left}\) ratio is low, i.e. the dominated input is launched into the CW modes through the left port, only small intensity variations are observed both at\(\omega\) and \(2\omega\) (Fig. 5a,d). In sharp contrast, much larger modulations are visible in both phase spectra when \({P}_{right}/{P}_{left}=0.45\). Particularly, a total annihilation point of SHG is observed in the CCW modes at the zero phase delay (Fig. 5b), when most of SHG occurs in a chiral manner in the other CW direction. This is caused by the destructive interference between the two inphase incident beams at \(\omega\) (Fig. 5e). Note that, the power ratio is not one, which is a prerequisite condition for a linear total destructive interference. Here it is mainly due to the asymmetrical scattering as mentioned above. Moreover, we notice unsynchronized phase modulations by comparing the two frequency spectra at \(\omega\) and \(2\omega\), this is caused by the nature of nonlinear second harmonic processes in which two fundamental photons are converted into one single secondharmonic photon, hence their phases are not synchronized[detailed theoretical calculation in the supplement]. With a higher ratio, i.e. \({P}_{right}/{P}_{left}=1.9\), we observe a reversal direction of SHG to the CCW direction when the incident waves are inphase, but the SHGs in both directions tend to be equal at a phase difference of \(\pi /2\). To demonstrate the chirality of SHGs during the phase modulation, we plot the distinction ratio of SHGs between the CW and CCW directions as opposed to the power ratio \({P}_{right}/{P}_{left}\) in Fig. 5 g. An optimal contrast point is evident near \({P}_{right}/{P}_{left}=0.45\) with a distinction ratio over 100 times (Fig. 5b), meaning SHGs are highly directional in the CW direction. Moving to either side, such distinction ratio diminishes. These results offer an attractive tool for unidirectional SHG and coherent controlled nonlinear processes in the future [35]. In addition, according to previous studies, we can use two nanotips introduced in the mode volume as two scatters[36] or etch holes in the microring[37] to break the chiral symmetry. Therefore, designing an asymmetric cavity for a secondharmonic generation with a high distinct ratio in the transparency state is feasible.
Conclusion
In summary, we experimentally demonstrate a selfinduced transparency effect in a perfectly absorbing optical microcavitybased second harmonic generator, which is capable of perfectly absorbing incoming waves in the linear regime, but turns into a transparency state and begins to emission second harmonics in a coherent controlled chiral manner. There are a few possible impacts on the optics fields and quantum physics. For example, the signature selfinduced transparency may partially resemble the nonlinear behavior of an electrical diode, a building block for the integration circuits (IC). Similar to the forwardbiased scenarios of the electrical diode, the signal transmission is relatively low with a small biased voltage, but nonlinearly and drastically increases with a larger voltage. Our device may serve as an optical version of the diode. The second feature of coherent controllable and chiral transparency may offer another opportunity for alloptical switching, just like its counter electrical transistors in IC. Moreover, the chiral emission of SHG is also an attractive platform for optical frequency conversion applications, in which the SHG usually copropagates with its pump beam due to the phasematching condition. Here in our device, we may specifically design the output port of the SHG, which may/may not align with its pump depending on the coherent control. At last, we believe these results are universal across multidiscipline in microwaves, acoustics, mechanics, and matter waves, hence it paves the way for practical applications of coherent control and nonlinear induced transparency in information processing and frequency conversion.
Methods
Sample fabrication
The microdisk resonator (~ 100 \(\mu\)m diameter) is fabricated with femtosecond laser direct writing and the chemicalmechanical(CM) polishing [38] in four steps. First, a thin layer of chromium (Cr) is deposited on the surface of the LNOI through thermal evaporation coating, then spaceselective femtosecond laser direct writing is used to pattern the Cr film into a circular disk, next, CM polishing is significant for improving the surface smoothness, leading to high Qfactor, finally, removing the SiO2 buffer layer and the Cr thin film with two consecutive chemical wet etching processes. The thickness of the sidewall of the microcavity is 900 nm and the typical Q factor is about 10^{6}, which leads to very strong local field strength. The tapered fiber is made of the standard singlemode fiber (G.652.D) and is melted by oxyhydrogen flame. In the coupling region, the tapered fiber is 2 ~ 3 \(\mu\)m in diameter and is in contact with the microdisk resonator for stability during the whole experiment.
Experimental details
A continuously tunable laser (CTL, Toptica Photonics) with a center wavelength of 1550 nm is used as the optical source. The optical source is amplificated by an EDFA and divided into two branches (CW and CCW) by the coupler (50:50). The intensity and polarization of the CW branch are controlled by the variable optical attenuator (VOA) and polarization controller (PC). The other branch (CCW) is modulated by an electrooptic modulator (EOM) to vary relative phase between two branches. Two power meters are used to monitor the input power of each branch[see Supplementary S5], Once the pump is detuned at the required frequency, the relative phase is changed by EOM using an external control signal.
Fundamental and secondharmonic signal detection
The SH signal is detected by a photomultiplier tube (PMT, CR114) connected to an OSA and the transmission spectra of each branch are detected by two PDs (DET02AFC) [see Supplementary S5]. There is no need to use the filter in this system. Because the PMT does not respond to the 1,550 nm communication band and the response band of DET02AFC is 8001700 nm, not including 775 nm. The SH signal is detected from the \(1\times 2\) coupler (50:50) and the transmission signal of the pump is detected from a \(2\times 2\) coupler (10:90) through 10% end in each branch. The external control signal is a triangular wave with 20 Vpp and 1 kHz frequency and was used as a trigger source in OSA during this experiment.
Critical coupling and perfect absorption condition
Critical coupling occurs when the external lifetime is matched to the intrinsic cavity decay rate \(\left({\tau }_{ex}^{1}={\tau }_{0}^{1}\right)\) i.e. the coupling strength between waveguide and microcavity is equal to the intrinsic loss of the cavity \({\gamma }_{c1}={\gamma }_{1}\). In this case, the transmission past microcavity vanishes, and entire power is transferred from the optical wave to the cavity modes. The transmission vanishes due to the interference of the cavity leakage field and transmitted pump field, which exhibit equal magnitude but a relative phase shift \(\pi\). This completely destructive interference is also called perfect absorption. To achieve perfect absorption, it is necessary to appropriately choose the values of the system parameters, such as the gap distance between waveguide and cavity, the scattering strength. In addition, the intensities and relative phases of the input beams are significant as well. In our experiment, we accurately control the coupling strength \({\gamma }_{c1}\) by a 3axis nanotranslation stage (Thorlabs, MDT630B). We first set the gap distance between waveguide and cavity equal to 500 nm, then reduce the distance slowly, until reaches critical coupling condition.
Phase control
The total relative phase is defined as\(({\varphi }_{2}{\varphi }_{1}\pi /2{\Delta }\phi )\) is influenced by two factors [see supplementary S2]. One is the constant phase results from the structure of the system, which determines the output intensity relationship between two ports (Fig. 4cf). This phase is related to the coupling strength \({\gamma }_{c1}\), intrinsic loss of the cavity \({\gamma }_{1}\) and the detuning \({\varDelta }_{1}\). In this experiment, the coupling condition is fixed, so we change the constant phase by varying \({\varDelta }_{1}\). The other is phase difference \(\left({\Delta }\phi \right)\) between two branches, controlled through EOM. The range of \({\Delta }\phi\) is from 0 to \(2\pi\) scanned by an external triangle signal source (1 kHz,20Vpp). The output intensity changes as the relative phase changes due to interference.
Data Availability
The data that support the findings of this study are available from the authors on reasonable request.
Abbreviations
 CPA:

Coherent perfect absorber.
 EIT:

electromagnetically induced transparency.
 SHG:

Second harmonic generation.
 FW:

Fundamental wave.
 CW:

clockwise.
 CCW:

counterclockwise.
 IC:

integration circuits.
References
Chong YD, Ge L, Cao H, Stone AD. Coherent perfect absorbers: timereversed lasers. Phys Rev Lett. 2010;105:053901.
Wan W, Chong YD, Ge L, Noh H, Stone AD, Cao H. Timereversed lasing and interferometric control of absorption. Science. 2011;331:889–92.
Landy NI, Sajuyigbe S, Mock JJ, Smith DR, Padilla WJ. Perfect metamaterial absorber. Phys Rev Lett. 2008;100:207402.
Mei J, Ma G, Yang M, Yang Z, Wen W, Sheng P. Dark acoustic metamaterials as super absorbers for lowfrequency sound. Nat Commun. 2012;3:756.
Ma G, Yang M, Xiao S, Yang Z, Sheng P. Acoustic metasurface with hybrid resonances. Nat Mater. 2014;13:873–8.
Andreas M, Bodhaditya S, Christian B, Jian J, Jens B, Ralf L, Zezyulin DA, Konotop VV, Herwig O. Coherent perfect absorption of nonlinear matter waves. Sci. Adv. 2018;4:8.
Zheng Y, Yang J, Shen Z, Cao J, Chen X, Liang X, Wan W. Optically induced transparency in a microcavity. Light Sci Appl. 2016;5:e16072.
Kats MA, Capasso F. Optical absorbers based on strong interference in ultrathin films. Laser Photon Rev. 2016;10:735–49.
Konstantatos G, Sargent EH. Nanostructured materials for photon detection. Nat Nano. 2010;5:391–400.
Liu N, Mesch M, Weiss T, Hentschel M, Giessen H. Infrared perfect absorber and its application as plasmonic sensor. Nano Lett. 2010;7:2342–8.
Mostafazadeh A. Nonlinear spectral singularities for confined nonlinearities. Phys Rev Lett. 2013;110:260402.
Suwunnarat S, Tang Y, Reisner M, Mortessagne F, Kuhl U, Kottos T. Nonlinear coherent perfect absorption in the proximity of exceptional points. Commun Phys. 2022;5:5.
Boller KJ, Imamoğlu A, Harris SE. Observation of electromagnetically induced transparency. Phys Rev Lett. 1991;66:2593–6.
Harris SE, Yamamoto Y. Photon switching by quantum interference. Phys Rev Lett. 1998;81:3611–4.
Hau LV, Harris SE, Dutton Z, Behroozi CH. Light speed reduction to 17 metres per second in an ultracold atomic gas. Nature. 1999;397:594–8.
Phillips DF, Fleischhauer A, Mair A, Walsworth RL, Lukin MD. Storage of light in atomic vapor. Phys Rev Lett. 2001;86:783–6.
Zhang F, Feng Y, Chen X, Ge L, Wan W. Synthetic antiPT symmetry in a single microcavity. Phys Rev Lett. 2019;124:053901.
Qin T, Yang J, Zhang F, Chen Y, Shen D, Liu W, Chen L, Jiang X, Chen X, Wan W. Fastand slowlightenhanced light drag in a moving microcavity. Commun Phys. 2020;3:118.
Xu Q, Sandhu S, Povinelli ML, Shakya J, Fan SH, Lipson M. Experimental realization of an onchip alloptical analogue to electromagnetically induced transparency. Phys Rev Lett. 2006;96:123901.
Yanik MF, Suh W, Wang Z, Fan SH. Stopping light in a waveguide with an alloptical analog of electromagnetically induced transparency. Phys Rev Lett. 2004;93:233903.
Zhang S, Genov DA, Wang Y, Liu M, Zhang X. Plasmoninduced transparency in metamaterials. Phys Rev Lett. 2008;101:047401.
Mccall S, Hahn E. SelfInduced Transparency. Phys Rev. 1969;183:457–85.
Slusher RE, Gibbs HM. SelfInduced Transparency in Atomic Rubidium. Phys Rev A. 1972;5:1634.
Cai M, Painter O, Vahala KJ. Observation of Critical Coupling in a Fiber Taper to a SilicaMicrosphere WhisperingGallery Mode System. Phys Rev Lett. 2000;85:74.
Zhu D, Shao L, Yu M, Cheng R, Desiatov B, Zhang M, Lončar M, et al. Integrated photonics on thinfilm lithium niobate. Adv Opt Photon. 2021;13:242–352.
Carmon T, Yang L, Vahala KJ. Dynamical thermal behavior and thermal selfstability of microcavities. Opt Express. 2004;12:4742–50.
Wong ZJ, Xu YL, Kim J, O’Brien K, Wang Y, Feng L, Zhang X. Lasing and antilasing in a single cavity. Nat Photon. 2016;10:796–801.
Jalas D, Petrov A, Eich M, Freude W, Renner H. What is — and what is not — an optical isolator. Nat Photon. 2013;7:579–82.
Wiersig Jan. Structure of whisperinggallery modes in optical microdisks perturbed by nanoparticles. Phys Rev A. 2011;84:063828.
Wiersig Jan. Enhancing the Sensitivity of Frequency and Energy Splitting Detection by Using Exceptional Points: Application to Microcavity Sensors for SingleParticle Detection. Phys Rev Lett. 2014;112:203901.
Sweeney WR, Hsu CW, Rotter S, Stone AD. Perfectly Absorbing Exceptional Points and Chiral Absorbers. Phys Rev Lett. 2019;122:093901.
Peng B, Zdemir AK, Liertzer M, Chen W, Yang L. Chiral modes and directional lasing at exceptional points. Proc. Natl. Acad. Sci. U.S.A. 2016;113:6845–6850.
Soleymani S, Zhong Q, Mokim M, Rotter S, ElGanainy R, Ozdemir SK. Chiral coherent perfect absorption on exceptional surfaces. Nat Commun. 2022;13:599.
Snijder HJ, Frey JA, Norman J, Flayac H, Savona V, Gossard AC. Observation of the unconventional photon blockade. Phys Rev Lett. 2018;121:043601.
Yang J, Yuan L, Qin T, Zhang F, Chen Y, Jiang X, Chen X, Fan SH, Wan W. Phononinduced anomalous gauge potential for photonic isolation in frequency space. Optica. 2021;8:1448–57.
Zhu J, Özdemir SK, He L, Yang L. Controlled manipulation of mode splitting in an optical microcavity by two Rayleigh scatterers. Opt Express. 2010;18:23535–43.
Gao G, Zhang Y, Zhang H, Wang Y, Huang Q, Xia J. Airmode photonic crystal ring resonator on silicononinsulator. Sci Rep. 2016;6:19999.
Wu R, Zhang J, Yao N, Fang W, Qiao L, Chai Z, Lin J, Cheng Y. Lithium niobate microdisk resonators of quality factors above 10^{7}. Opt Lett. 2018;43:4116–9.
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Funding
This work was supported by the National Science Foundation of China (Grant No. 92050113, No. 12274295, No. 11304201); National key research and development program (Grant No. 2016YFA0302500, 2017YFA0303700); Shanghai MEC Scientific Innovation Program (Grant No. E00075).
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W.W. initiated the idea; W.W., Y. C. designed the study; L.G. performed the theoretical study; W.W., Y. C, Y. Z, X.C. supervised the work; J. H. performed experimental work; J. L., J. Z. fabricated the devices; G. Z., Y. C., F. Z. analyzed the data; W.W., Y. C. wrote the paper; All authors reviewed the manuscript.
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Hou, J., Lin, J., Zhu, J. et al. Selfinduced transparency in a perfectly absorbing chiral secondharmonic generator. PhotoniX 3, 22 (2022). https://doi.org/10.1186/s4307402200068y
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DOI: https://doi.org/10.1186/s4307402200068y
Keywords
 CPA
 Microresonator
 Selfinduced transparency
 Chiral
 SHG