Abstract
The nonlinear scattering of a linear optical wave from a conservative soliton has been widely studied in optical fibers as a mechanism for nonlinear frequency conversion. Here we extend this analysis to consider the scattering of an externally injected probe wave from a dissipative cavity soliton circulating in a Kerr microresonator. We demonstrate, both theoretically and experimentally, that this nonlinear interaction can be harnessed for useful expansion of the soliton frequency comb via the formation of a secondary idler comb. We explore the physics of the process, showing that the phase detuning of the injected probe from a cavity resonance plays a key role in setting the central frequency of the idler comb, thus providing a convenient parameter through which to control the spectral envelope of that comb. Our results elucidate the dynamics that govern the interactions between dissipative Kerr cavity solitons and externally injected probe waves, and could prove useful in the design of future Kerr frequency comb systems by enabling the possibility to provide highpower comb lines in a specified spectral region simply through the injection of a suitably chosen probe.
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Introduction
Microresonator frequency combs (microcombs) offer an attractive pathway towards the realization of miniaturized, lowpower coherent optical frequency combs^{1,2,3}. Applications of these chipscale devices have already been demonstrated across fields ranging from telecommunications^{4} and spectroscopy^{5} to remote sensing^{6,7} and medical diagnostics^{8}. In the vast majority of systems, the resonators are driven with a monochromatic laser, and frequency combs form through the thirdorder optical Kerr nonlinearity^{1}. In such systems, coherent comb states are underpinned by the excitation of ultrashort localized structures known as temporal cavity solitons^{9} – also referred to as dissipative Kerr solitons^{2,10}.
The spectral properties of Kerr microcombs are dominantly set by the material and geometric parameters of the microresonator. A key comb property is its spectral bandwidth, which (to leadingorder) scales as^{11}
where γ, \({{{{{{{\mathcal{F}}}}}}}}\), and β_{2} are the resonator’s Kerr nonlinearity coefficient, finesse, and groupvelocity dispersion (GVD) at the driving wavelength, and P_{in} is the driving power, respectively. The large \({{{{{{{\mathcal{F}}}}}}}}\) and γ of microresonators are thus highly conducive to the realization of combs with large spectral bandwidth. In addition, the dispersion of microresonators can be engineered to provide further increase in the attainable comb bandwidth. This typically involves both lowering the resonator’s GVD coefficient ∣β_{2}∣, and optimizing its thirdorder dispersion so as to allow additional spectral extension through the formation of dispersive waves that are phasematched to the pump^{12,13,14}.
Very recently, a new approach has been put forward that allows for the spectral characteristics and extent of microcombs to be controlled even after the fabrication of the resonator (whereupon its material and geometric properties are set). Specifically, the injection of a frequencyshifted probe field alongside the main comb generating pump has been shown to permit controllable expansion of the comb spectrum via two distinct mechanisms^{15,16,17}. In the first mechanism^{15,16}, a cavity soliton excited by the pump field imparts a nonlinear phase shift on the intracavity field of the frequencyshifted probe. This induces a frequency comb structure around the probe frequency via crossphase modulation (XPM). In the second mechanism, frequency components of the soliton comb are spectrally translated through the fourwavemixing process of nonlinear Bragg scattering^{17}, again giving rise to a comb structure around the frequencyshifted probe field. Both mechanisms result in the generation of a secondary comb around the probe frequency, with line spacing equal to the spacing of the original soliton comb, yet they rely on fundamentally different physical phenomena: incoherent XPM^{15,16} and coherent Bragg scattering^{17}.
Recent experiments have unequivocally demonstrated the application potential of Braggscattering spectral expansion: a coherent Kerr microcomb with an expanded bandwidth of 1.6 octaves was reported in^{17}. However, a number of questions remain open with regards to the physics that underpin the phenomenon. For instance, earlier studies^{18,19} have shown that nonlinear Bragg scattering of a frequency comb can be understood as the frequencydomain description of a particular solitonlinear wave interaction^{20,21,22,23} that has been extensively studied in the context of conservative (singlepass) nonlinear fibre optics^{24,25,26,27}. This raises the question as to whether the simple phasematching conditions known to govern the process in the singlepass case hold predictive power in the resonator context. In addition, nonlinear Bragg scattering is intrinsically a coherent FWM (fourwave mixing) process, and could therefore be envisaged to depend upon the linear detuning of the probe wave from a cavity resonance; however, no discussion of the role of detuning has hitherto been presented.
Here we theoretically and experimentally study the spectral extension of soliton microcombs via coherent FWM Braggscattering. We show that the simple phasematching condition that underpins solitonlinear wave interactions in singlepass systems^{19} remains valid in the resonator context, provided however that the phase detuning of the probe wave is appropriately accounted for. Indeed, we find that this detuning plays a key role in the process, providing a convenient parameter through which to control the spectral characteristics of the comb extension. We perform experiments in a magnesiumfluoride (MgF_{2}) microdisk resonator, and demonstrate the generation of frequency tunable, lownoise idler combs that possess identical line spacing, and the same lownoise characteristics, as the driving cavity soliton comb. We further highlight the flexibility of this comb expansion technique by swapping the spectral locations of the cavity soliton pump and the probe wave whilst still maintaining the required phasematching – and hence comb extension. Our results provide significant insights into the spectral extension of soliton microcombs, and highlight the intimate linkage between Bragg scattering spectral extension and solitonlinear wave interactions that have been studied widely in the context of nonlinear fiber optics and supercontinuum generation^{18,19,20,21,22,23,24,25,26,27}. Whilst our experimental results are obtained in a monolithic crystalline microresonator we expect these results to find useful application across all microresonator platforms.
Results
Soliton linearwave scattering
We begin by briefly recounting how interactions between solitons and weak linear waves can enact resonant energy transfer to new frequencies in Kerr media^{20,21,22,23,28,29,30,31}. Considering a superposition field E = S + p, where S and p represent the soliton and the probe, respectively, the Kerr nonlinearity ∣E∣^{2}E will after linearization with respect to p yield three terms: \({\leftS\right}^{2}S\), \(2{\leftS\right}^{2}p\), and S^{2}p^{*}. Each of these three terms can drive resonant energy transfer to new waves^{30}, provided that those waves are phasematched to one of the driving terms. In fact, the first term is responsible for the generation of the standard dispersive waves that are directly phasematched with the soliton^{28,29}. On the other hand, the second and third terms represent nonlinear mixing between the soliton and the weak probe wave, and can drive additional phasematched radiation processes^{20,21,22,23,31}. In particular, the \(2{\leftS\right}^{2}p\) interaction has been shown to drive both the incoherent XPM and coherent FWM Bragg scattering interactions^{22}.
Earlier studies have shown that the solitonlinear wave interaction can be understood in the frequency domain as a cascade of individual FWM Bragg scattering processes^{18,19}. Specifically, pairs of discrete frequency components of a periodic train of solitons can act as pumps that drive a Bragg scattering cascade that translates the incident linear wave to a new idler frequency [see Fig. 1(a), (b)]. Remarkably, this cascade can be phasematched even though none of the elementary FWM processes are phasematched^{18,19,32}; moreover, the phasematching condition of the entire cascade is (approximately) the same as that of the solitonlinear wave interaction driven by the nonlinear polarization term \(2{\leftS\right}^{2}p\). In what follows, we show that this result extends to resonator configurations by demonstrating that the spectral extension of soliton microcombs via FWM Bragg scattering obeys the phasematching condition of the pertinent timedomain solitonlinear wave interaction.
Soliton linearwave phasematching
To derive the solitonlinear wave phasematching condition in a resonator configuration, we note that the phase accumulated by the linear idler wave at frequency ω_{i} over one round trip is: ϕ_{i} = β(ω_{i})L − ω_{i}t_{R}, where β(ω), L, and t_{R} are respectively the propagation constant, length, and round trip time of the resonator. Phasematching is achieved when ϕ_{i} = ϕ_{p} + 2πm, where ϕ_{p} = − ω_{p}t_{R} is the phase accumulated by the externallyinjected probe wave (at the input to the resonator) and m is an integer^{33}. Expanding the propagation constant β(ω) as a Taylorseries around the soliton pump, ω_{s}, we obtain
where δ_{p} is the phase detuning of the injected probe from the cavity resonance closest to it, and the reduced dispersion
The coefficient q = m − m_{0} with m_{0} the mode index of the resonance closest to ω_{p} describes phasematching to higherorder resonant sidebands that will not be considered in this work; in what follows, we set q = 0. We note that the analysis presented above considers only linear contributions to the idler’s phasematched frequency. Cross phase modulation between the idler wave and the other intracavity fields present will contribute an additional nonlinear contribution to this shift^{14,34}. The magnitude of this nonlinear shift can be estimated by comparing the difference between the idler frequency shift obtained from a generalized LugiatoLefever equation (LLE) simulation that includes all nonlinear contributions (see Methods) and that predicted by Eq. (2). For the experimental parameters used in this work, we find the difference between these two values to be only of the order of a few percent. For this reason we omit these terms from our phasematching analysis.
Equation (2) is akin to the phasematching condition for Braggtype solitonlinear wave interactions in singlepass fibre configurations^{19}, but with the additional probe detuning δ_{p} accounting for the resonant nature of the system. Importantly, the presence of δ_{p} significantly relaxes the phasematching requirements: whilst higherorder dispersion is required in singlepass configurations, in resonators phasematching can be achieved even with a purely quadratic dispersion profile [see Fig. 1(c), (d)]. Explicitly, for a resonator with secondorder dispersion only, the (angular) frequency detuning Ω_{i} = ω_{i} − ω_{s} of the newly generated idler field from the soliton pump satisfies:
where Ω_{p} = ω_{p} − ω_{s}. It is worth noting that Eq. (5) predicts two phasematched idler frequencies symmetrically located either side of the cavity soliton pump. However, the FWM Bragg cascade to the idler frequency located on the opposite side of the cavity soliton to the probe will require a cascade with substantially more steps and hence be less efficient. Indeed, for the parameters used in this paper, only the idler frequency closest to the probe frequency is observed in simulations and experiments. For different resonator parameters, however, it may be possible to efficiently drive both cascades resulting in new spectral components generated on both sides of the cavity soliton^{17}.
Illustrative simulations
To confirm the analysis above, we performed numerical simulations using the generalized LLE (see Methods), and compared the simulations to predictions based on Eq. (5). Figure 2 shows results from simulations that use parameters similar to the experiments that will follow (see figure caption). In particular, the false colour plot in Fig. 2(a) shows the spectral envelope of the intracavity field as a function of the probe phase detuning δ_{p} normalized to the resonance halfwidth (Δ_{p} = δ_{p}/α), where α corresponds to half the intracavity power lost per roundtrip. To obtain this plot, at each probe detuning a cavity soliton is first excited (at Ω = ω − ω_{s} = 0) and allowed to stabilize before the probe field is turned on. Also, in Fig. 2(c)–(f) we show lineplots of selected spectra in more detail, whilst Fig. 2(g)–(j) show the corresponding temporal intensity profile of the intracavity field over a single roundtrip.
In addition to the broadband soliton field around Ω = 0 and the injected probe field at Ω_{p}, a third wave whose position changes continuously with the probe detuning is clearly visible. This corresponds to the idler comb that is generated via the solitonlinear wave interaction described above. Indeed, in Fig. 2(b) we plot the peak frequency shift of the idler comb as a function of the probe detuning, superimposed with the theoretical prediction of the phasematched frequency given by Eq. (5). The agreement between the simulated idler frequency and the theoretical prediction is very good, validating the use of the linearised phasematching expression of Eq. (5) for our experimental parameters. When the probe detuning is sufficiently close to its own resonance [with Δ_{p} ∈ ( − 3, 11)], our simulations predict that the solitonlinear wave interaction is interrupted. This occurs because the probe itself undergoes modulation instability within this range of detunings, as clearly evidenced by the characteristic modulation instability spectral features observed in Fig. 2(a). For most detunings within this range, the large intensity fluctuations of modulation instability prevent the persistence of the cavity soliton altogether^{39,40} and accordingly prohibit any solitonlinear wave interaction. However, for a narrow sliver of detunings [with Δ_{p} ∈ ( − 3, 1)], our simulations predict that the cavity soliton can coexist with the modulation instability state associated with the probe, and in this case a linear wave interaction can take place, but with the noise from the probe’s modulation instability transferred to both the soliton and the idler combs, resulting in lowcoherent states. This noiselike modulation instability structure can be clearly seen in the spectral and temporal traces obtained at Δ_{p} = − 1 plotted in Fig. 2(d), (h). The incoherence arising from modulation instability is in stark contrast with the results seen at the other detunings shown in Fig. 2(c, g), (e, i) and (f, j). Here, simulations confirm that both the soliton and idler combs are coherent as required for useful spectral extension, and stable temporal structures are observed with the newly generated idler wave manifesting itself in the time domain as an oscillatory tail on the soliton’s leading edge. At this point, we note that the simulations presented here consider equal driving powers for the soliton and external probe fields. Simulations and theoretical considerations show that the efficiency of the solitonlinear wave cascade is set by the soliton pump power only^{18}. Varying the external probe power will thus result in the power in the idler comb simply scaling proportionally. The exact value of probe power used does, however, play an important role in the range of probe detunings Δ_{p} over which modulation instability is observed in the probe field, with larger probe powers resulting in wider regions of modulation instability.
Experiments
For experimental demonstration, we use a setup that is built around an MgF_{2} microdisk with a free spectral range (FSR) of 58.4 GHz (see Methods) ^{41,42,43}. The microdisk is driven by three continuouswave lasers: A Cband pump laser at 1550 nm, an Lband pump laser 1582 nm, and a third laser at 1534 nm configured to act as an auxiliary pump that provides thermal compensation during the cavity soliton excitation^{44,45}. The two pump lasers are coupled to the same mode family, and they can interchangeably act as the solitongenerating pump and the probe field. The auxillary laser (wavelength fixed at 1534 nm) is coupled to a different modefamily of the resonator to ensure it does not participate in the solitonlinear wave dynamics.
We first set the wavelength of the Lband pump to 1582 nm and excite a cavity soliton at that wavelength. The remaining Cband laser acts the probe, and is tuned into resonance close to 1550 nm from the bluedetuned (negative Δ_{p}) side. Figure 3(a)–(c) show the comb spectra measured at the output of the resonator as the probe detuning is scanned into resonance. We can clearly observe an idler peak that moves towards the probe as the detuning Δ_{p} is increased. The idler peak tunes continuously until we reach the modulation instability region of the probe field, at which point the cavity soliton ceases to exist and the solitonlinear wave interaction is halted – in accordance with our simulations [see Fig. 2(a), (b)]. We then reset the experiment such that a new cavity soliton is excited at 1582 nm, and tune the probe field into resonance from the reddetuned (positive Δ_{p}) side. Figure 3(d)–(f) show the resulting spectra, and we again observe the appearance of an idler peak that continuously tunes towards the probe, now as Δ_{p} is decreased. These results are in qualitative agreement with the phasematching prediction of Eq. (5), with positive (and negative) probe detunings observed to generate idler peaks at frequencies that are below (and above) the original probe frequency.
Figure 3 (g)–(l) show the lowfrequency RF (radio frequency) spectra of each microcomb state shown in Fig. 3(a)–(f). All of the spectra are clean with no excess noise, indicating that we are indeed observing lownoise, stable frequency combs. Yet, each RF spectrum does exhibit a single sharp RF tone. This is because, whilst the idler comb inherits the line spacing of the soliton comb, the two are offset from one another [see Fig. 1(b)], resulting in beating between adjacent lines in the region where the combs overlap. The beat frequency dν corresponds to the separation between the probe frequency and the soliton comb line closest to it. This can be written in terms of the soliton and probe detunings and the dispersive shift of the probe resonance as:
In our experiments, the RF beat tones range from 30 to 140 MHz, and are hence far too small to be resolved optically. Indeed, the optical comb spectra shown in Fig. 3 were recorded at an optical spectrum analyzer (OSA) resolution of 5 GHz, and a careful examination of these traces reveals only a single set of equispaced comb lines. Likewise, further RF intensitynoise measurements made using an electronic spectrum analyzer reveal only a lownoise background out to a frequency of 10 GHz (in addition to the lowfrequency RF beatnotes already observed in Fig. 3). Combined, these measurements confirm that the output spectrum is indeed composed of two individual lownoise combs: the first, the cavity soliton comb, and the second, the idler comb extending from the probe frequency to the phasematched idler peak, and spectrally offset from the cavity soliton comb.
The ability to measure the RF beat frequency between the soliton and the idler comb allows the two combs to be “stitched” together, i.e., the absolute frequencies of the idler comb lines to be directly related to the frequencies of the cavity soliton comb. In addition, when combined with measurements of the spectral position of the idler wave, the beat frequencies allow us to accurately estimate the parameters of the entire experiment (see Methods). Using parameters obtained in this manner (see caption of Fig. 2) in LLE simulations, we find excellent agreement with our experiments, as shown by the orange solid curves in Fig. 3(a)–(f). We observe particularly how the position and magnitude of the newly generated idler combs are very well reproduced by the simulations, and we also note that the idler positions are well predicted by the phasematched frequency given by Eq. (5).
The soliton and probe fields are interchangeable: we can exchange their roles by selecting appropriate detunings and still generate a phasematched idler comb. To show this, we set the detuning of the 1550 nm laser such that it generates a cavity soliton, and use the 1582 nm laser as the external probe. Figure 4(a)–(c) show the output comb spectra as the probe field is continuously tuned into resonance from the bluedetuned (i.e., negative Δ_{p}) side, whilst Fig. 4(d)–(f) show the corresponding RF spectra. The observed spectra are qualitatively identical to those obtained when the 1582 nm pump generates the cavity soliton. Moreover, we again find excellent agreement between the experimentally recorded spectra and the numerical results obtained from the LLE (red traces). The only adjustment to the simulation parameters used in Figs. 2 and 3 was a change to the value of the groupvelocity dispersion coefficient β_{2} = − 2.9 × 10^{−27}s^{2}m^{−1} due to the change in pump wavelength and residual thirdorder dispersion. The small spectral features visible in the experimentally measured spectra at ~1505 and 1515 nm are a result of mode crossings at these wavelengths^{46}. They play no significant role in the solitonlinear wave interaction and are not seen in our LLE simulations that considers only a single resonator mode family. Finally, we note in closing this section that for all the results presented here, the idler comb remains spectrally offset from the soliton comb (δν ≠ 0). It is possible to envisage different experimental conditions where δν could be set to zero. In this case, one would observe an interference between the contributions of the soliton and idler waves at each individual comb line. As the two lasers used to generate the soliton and probe driving fields are freerunning independent lasers, this interference would be expected to vary on the timescale set by the two lasers’ coherence times.
The results presented in Figs. 3 and 4 offer strong experimental support for the solitonlinear wave phasematching theory presented in the previous section. In addition to dynamics involving a single cavity soliton and the probe wave, our experiments show that more complex interactions can also take place. First, the solitonlinear wave interaction can occur when the resonator hosts several solitons. Indeed, in Fig. 5(a) we show comb spectra recorded at the resonator output with two temporally separated cavity solitons centred around a 1550 nm pump interacting with a probe field at 1582 nm; Fig. 5(b) shows the corresponding spectrum with the roles of the solitongenerating pump and the probe reversed. In both cases, a strong spectral modulation with a period of 4 nm can be observed, indicating the presence of two cavity solitons in the cavity separated by 2 ps. This spectral modulation manifests itself across both the cavity soliton and the idler combs, thus providing further evidence that the two combs are temporally locked to each other. Also shown in Fig. 5(a), (b) are theoretical \({{{{{\rm{sech}}}}}}^{2}\) profiles of the cavity soliton spectral envelope in the absence of the probe wave. This shows how the solitonlinear wave interaction leads to a substantial increase in comb intensity around the probe. Finally, in accordance with the simulations shown in Fig. 2, our experiments show that a narrow region of probe detunings exist where the probe can undergo modulational instability whilst still allowing the cavity soliton and the idler comb to persist. Figure 5(c) shows the measured optical spectrum recorded in this regime, superimposed with corresponding simulations, and we indeed observe characteristic (i) modulation instability sidebands around the 1550 nm probe wavelength and (ii) soliton \({{{{{\rm{sech}}}}}}^{2}\) profile around the 1582 nm cavity soliton pump. Moreover, the RF spectrum of this state [see Fig. 5(d)] shows clearly elevated level of intensity noise, as expected due to the chaotic nature of the modulation instability state.
Conclusion
To summarize, we have shown that the nonlinear interaction between a cavity soliton and an externally injected probe can engender spectral extension of a Kerr microcomb via the formation of a secondary idler comb. We have shown that the process is underpinned by a simple phasematching condition derived from the timedomain solitonlinear wave interaction picture, revealing that the probe field’s linear detuning plays a key role in controlling the phasematched frequency – and hence the spectral characteristics of the idler comb. We obtain a simple linear phasematching expression for the frequency shift of the phasematched idler wave and find that, for our parameters, it agrees well with the numerical shifts predicted by a full LLE simulation. The idler and its generating soliton comb have the same line spacing and lownoise characteristics, but are spectrally offset from one another; measurement of the RF beat frequency between the two combs allows the frequencies of the idler comb lines to be directly related to the cavity soliton comb. Combined, these properties make solitonlinear wave scattering an attractive candidate for the spectral expansion of Kerr combs, enabling comb power to be enhanced at desired spectral locations simply through the injection of an appropriate external probe field. We anticipate this ability could find useful application in many areas of microcomb research, including spectroscopy, frequency metrology and optical frequency synthesis. Finally, we close by emphasizing that the solitonlinear wave interaction described in our work represents the timedomain description of cascaded FWM Bragg scattering^{18,19}, which has been linked to microcomb spectral extension in recent works completed in parallel with our study^{17}.
Methods
Experimental setup
Our setup is built around an MgF_{2} microdisk shaped via diamond point turning and then handpolished to achieve a measured finesse of \({{{{{{{\mathcal{F}}}}}}}}\approx 3.1\times 1{0}^{4}\) at 1550 nm. The disk has a minor radius of 30 μm, and a major radius of 600 μm, yielding an freespectral range of 58.4 GHz. A micron diameter fiber taper is used to couple the driving fields to and from the resonator. The microdisk is driven by three optical fields derived from two Cband externalcavitylasers (ECL), and one Lband ECL. Each laser is amplified by an erbiumdopedfiber amplifier, then filtered and coupled to the optical taper using fiber wavelengthdivisionmultiplexers. One of the Cband lasers and the Lband laser are coupled to the same mode family, and they can interchangeably act as the solitongenerating pump and the probe field. The remaining Cband laser (wavelength fixed at 1534 nm) is coupled to a different modefamily of the resonator and configured to act as an auxiliary pump that provides thermal compensation during the cavity soliton excitation. Throughout our measurements, the powers of the soliton and probe lasers were set to 80 mW whilst that of the auxiliary pump was set to 150 mW.
Bichromaticallypumped LLE Simulations
Our experimental observations are modelled by the LugiatoLefever equation (LLE)^{15,35,36,37,38}:
Here E(t, τ) describes the slowlyvarying intracavity electric field envelope, t is a “slow” time that describes the evolution of E(t, τ) at the scale of the photon lifetime, τ is a corresponding “fast” time that describes the envelope’s profile over a single roundtrip, \(\alpha =\pi /{{{{{{{\mathcal{F}}}}}}}}\) is half of the power lost per round trip (and equal to the resonance halfwidth), δ_{s} is the phase detuning of the solitongenerating pump from the cavity resonance closest to it, and θ is the input power coupling coefficient. The driving field E_{in}(t, τ) accounts for the bichromatic pumping and is defined as
where E_{in,s} and E_{in,p} are the pump amplitudes with units of W^{1/2} at the soliton and probe frequencies ω_{s} and ω_{p}, respectively. All simulation results presented in the paper were obtained by numerically integrating Eq. (7) using the splitstep Fourier method with parameters quoted in the caption of Fig. 2 (or elsewhere in the main text).
Fitting procedure
The following describes the procedure used to fit our simulations to our experimental data, allowing direct comparisons to be drawn. First, the change in probe detuning between each spectrum (shown in Fig. 2) can be calculated from the change in the measured RF beat notes, Δdν, as Δδ_{p} = 2π ⋅ (Δdν/FSR); second, the GVD coefficient β_{2} can be extracted by fitting the change in idler position with the change in probe detuning: \({{\Delta }}{\Omega }_{{{{{{{{\rm{i}}}}}}}}}={({\beta }_{2}L{{{\Omega }}}_{{{{{{{{\rm{i}}}}}}}}})}^{1}{{\Delta }}{\delta }_{{{{{{{{\rm{p}}}}}}}}}\); third, γ and δ_{s} can be estimated by fitting numerical simulations to the cavity soliton spectrum, and to the measured value of δ_{p} at which the probe undergoes modulation instability. These procedures yield the parameters quoted in the caption of Fig. 2.
Data availability
The data that support the findings of this study are available from the corresponding author upon reasonable request.
Code availability
The code that supports the findings of this study are available from the corresponding author upon reasonable request.
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Acknowledgements
This work was supported by the Marsden Fund and the Rutherford Discovery Fellowships of the Royal Society of New Zealand.
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P.C.Q. performed all the experiments. V.N. performed numerical modelling of resonators. F.A., L.S.T., and H.G.L.S. fabricated the resonators. M.E. and S.C. contributed to theoretical interpretation of the results. M.E. and S.G.M. wrote the manuscript. All authors contributed to discussing and interpreting the results.
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Communications Physics thanks Dmitry Skryabin, Naoya Kuse and Xingyuan (Mike) Xu for their contribution to the peer review of this work. Peer reviewer reports are available.
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Qureshi, P.C., Ng, V., Azeem, F. et al. Soliton linearwave scattering in a Kerr microresonator. Commun Phys 5, 123 (2022). https://doi.org/10.1038/s42005022009035
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DOI: https://doi.org/10.1038/s42005022009035
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