1 Introduction
An optical modulator [-23pc]controls the light amplitude or phase through the effects of electro-optics, acoustic-optics, thermos-optics or optic-optics[ Reference Kobayashi, Sueta, Cho and Matsuo 1 – Reference Alkeskjold, Lægsgaard, Bjarklev, Hermann, Anawati, Broeng, Li and Wu 6 ]. Optical modulators have been vital in optical signal processors, photonic integrated circuits and fiber optic communication networks[ Reference Wang, Zhang, Chen, Bertrand, Shams-Ansari, Chandrasekhar, Winzer and Lončar 7 – Reference Delmade, Krstić, Browning, Crnjanski, Gvozdić and Barry 9 ]. In particular, the combination of an intracavity optical modulator and a laser resonator has been routinely utilized for generating mode-locked lasers or optical frequency combs[ Reference Lee, Kim, Shin, Lee, Kim and Eom 10 – Reference Diddams, Ma, Ye and Hall 13 ]. Intracavity modulation can be achieved by saturable absorption[ Reference Saarinen, Lyytikäinen and Okhotnikov 14 ], χ(2)[ Reference Ricciardi, Mosca, Parisi, Leo, Hansson, Erkintalo, Maddaloni, De Natale, Wabnitz and De Rosa 15 – Reference Melkonian, Forget, Bretenaker, Drag and Rosencher 18 ] or χ(3) [ Reference Englebert, Arabí, Parra-Rivas, Gorza and Leo 19 ] nonlinear processes. Regardless of the type of optical modulator, an optical resonator is indispensable to establish the periodic feedback of gain/loss. It is a nontrivial task to achieve phase locking of many longitudinal modes and generate mode-locked lasers without a laser resonator.
In this paper, we propose a novel category of optical modulator based on the χ(2) parametric process, and theoretically demonstrate that such an optical modulator enables the direct generation and phase locking of multiple sidebands without the need for optical resonators. The optical setup of the proposed optical modulator looks almost the same as an optical parametric amplifier (OPA), which does not require any optical components other than a χ(2) medium (Figure 1(a)). However, its transfer function is fundamentally different from OPAs. Conventionally, OPAs are operated in the regime of either small-signal amplification (where pump depletion is negligible) or saturated amplification, wherein back-conversion is carefully avoided[ Reference Cerullo and Silvestri 20 ]. In these OPAs, the χ(2) parametric process cannot expand the signal bandwidth, and the signal waveform remains almost the same during amplification.
(a) Schematic of a χ(2)-based optical modulator that provides a reciprocal-type transfer function. It consists of an OPA that is pumped by a quasi-continuous-wave laser and seeded by an amplitude-modulated (AM) laser. The output signal waveforms A out(t) calculated for (b) a square-modulated seed signal A in(t) and for (c) a sinusoidal AM seed signal A in(t). Here, A p and A v denote the modulation peak and valley of a sinusoidal AM seed signal.
However, in our scheme, the OPAs are deliberately pushed into the regime of full-back-conversion. It is well known that for an amplitude-modulated (AM) seed signal, those modulation peaks with higher amplitude deplete the pump more quickly, so they switch into back-conversion earlier than those modulation valleys. We demonstrate that in the regime of full-back-conversion, the signal waveform A out(t ) evolves into exactly the reciprocal of the incident waveform A in(t). In other words, OPA acts as an optical modulator that provides a reciprocal-type transfer function. For a square-modulated seed signal, such a modulator acts as an optical inverter, which changes the ‘1’ amplitude levels into ‘0’, and vice versa (Figure 1(b)). In particular, the reciprocal of a sinusoidal AM waveform is a train of Lorentz-shaped pulses, wherein the pulse duration is significantly shorter than the modulation period of the incident AM waveform. This link promises to produce a picosecond pulse train directly from a sinusoidal AM laser without the need for an optical resonator.
The paper is organized as follows. Section 2 characterizes how the χ(2) parametric process enables a reciprocal-type transfer function and how such a transfer function results in sideband generation in the frequency domain, as well as how the phase of all the sidebands evolves, which changes from the disorder state to the phase locking state. Section 3 studies the temporal and spectral characteristics of the output ultrashort pulse train, as well as their dependencies on the parameters of the OPA and sinusoidal AM. Section 4 discusses the influences of the crystal dispersion and parametric super-fluorescence (PSF). Section 5 presents the conclusion.
2 Generation and phase locking of sidebands
To demonstrate the sideband generation and phase locking in the regime of full-back-conversion, we simulate the χ(2) parametric process within a periodically poled lithium niobate (PPLN) waveguide by solving the coupled-wave equations[ Reference Zhou, Ma, Wang, Yuan, Xie and Qian 21 ] under the slowly varying envelope approximation, as given by the following:
$$\begin{align}\begin{array}{l}\frac{\partial {A}_\mathrm{s}\left(z,t\right)}{\partial z}+\sum \limits_{{m}=1}^{\infty}\frac{{\left(-i\right)}^{m-1}}{m!}{k}_\mathrm{s}^{(m)}\frac{\partial^m{A}_\mathrm{s}\left(z,t\right)}{\partial {t}^m}=-i\frac{d(z){\omega}_\mathrm{s}}{n_\mathrm{s}{c}_0}{A}_\mathrm{p}\left(z,t\right){A}_\mathrm{i}^{\ast}\left(z,t\right){e}^{-i\Delta k\cdot z},\\ {}\frac{\partial {A}_\mathrm{i}\left(z,t\right)}{\partial z}+\sum \limits_{m=1}^{\infty}\frac{{\left(-i\right)}^{m-1}}{m!}{k}_\mathrm{i}^{(m)}\frac{\partial^m{A}_\mathrm{i}\left(z,t\right)}{\partial {t}^m}=-i\frac{d(z){\omega}_\mathrm{i}}{n_\mathrm{i}{c}_0}{A}_\mathrm{p}\left(z,t\right){A}_\mathrm{s}^{\ast}\left(z,t\right){e}^{-i\Delta k\cdot z},\\ {}\frac{\partial {A}_\mathrm{p}\left(z,t\right)}{\partial z}+\sum \limits_{m=1}^{\infty}\frac{{\left(-i\right)}^{m-1}}{m!}{k}_\mathrm{p}^{(m)}\frac{\partial^m{A}_\mathrm{p}\left(z,t\right)}{\partial {t}^m}=-i\frac{d(z){\omega}_\mathrm{p}}{n_\mathrm{p}{c}_0}{A}_\mathrm{s}\left(z,t\right){A}_\mathrm{i}\left(z,t\right){e}^{i\Delta k\cdot z},\end{array}\end{align}$$
where A s,i,p, ω s,i,p and n s,i,p are the complex envelops, carrier frequency and refractive index of the signal, idler and pump, respectively, d(z) = ±d eff is the nonlinear coupling coefficient of collinear PPLN with collinear geometry, which changes sign in each quasi-phase matching period[ Reference Gayer, Sacks, Galun and Arie 22 ], Δk = k p–k s–k i is the wave-vector mismatch and k (m) = ∂(m) k/∂ω (m) refers to the effects of mth-order dispersion. In our simulations, the pump laser adopts a 527 nm pulse of 10 ns in duration and I p = 100 MW/cm2 in intensity, which is below the damage threshold of PPLN[ 23 ]. The seed signal adopts a sinusoidal AM laser of 10 W/cm2, which contains an initial pair of sidebands at the frequency offset of ±Ω = ±40 GHz with respect to the center frequency line at λ s0 = 1030 nm. In the time domain, the seed signal exhibits an amplitude modulation characterized by a modulation frequency of Ω = 40 GHz and an extinction ratio (ER) of 30 dB. Here, the ER is defined by the intensity ratio between the modulation peak and valley. It is a critical parameter that determines how many sidebands can be produced in our scheme. Nowadays, commercial electric-optic modulators can easily achieve an ER of 30–40 dB[ 24 ]. Our scheme does not require a carrier-envelope stable phase of the pump and signal pulse. For clarification, the effects of medium dispersion and the super-fluorescence noise are excluded in this section, and will be discussed separately in Section 4.
It is known that in the χ(2) parametric process, the temporal shape and duration of the signal change significantly upon back-conversion[ Reference Zhou, Ma, Wang, Yuan, Xie and Qian 21 ]. Since the parametric wave-mixing is instantaneous, each temporal slice of an AM seed signal amplifies independent of the others and thus experiences a different regime of gain saturation. The modulation peaks deplete the pump more quickly than the valleys do. In our simulated case (Figure 2(a)), the modulation peaks maximally deplete the pump at a crystal length of L p = 12.8 mm and then fall into back-conversion, while the valleys take a longer crystal length of L v = 17.7 mm before switching into back-conversion. After a certain crystal length, the amplitude of the incident valleys surpasses that of the incident peaks. This implies that the incident peaks evolve into valleys, while the valleys evolve into peaks.
(a) Amplitude evolution of the incident modulation peak (solid line) and valley (dotted line) versus the crystal length. (b) Amplitude evolution of the first five orders of sidebands A (n), where n refers to the order for each sideband.
The initial amplitude ratio between the modulation peaks (A
p) and valleys (A
v) is determined by the ER as
${A}_\mathrm{p}/{A}_\mathrm{v}=\sqrt{\mathrm{ER}}$
. When the incident peaks (valleys) turn into valleys (peaks), the intensity ratio between the initial peaks and valleys transfers to the reciprocal of the initial value with a crystal length of L
v < L < 2L
p according to Figure 2(a). For a temporal AM signal, this amplitude relationship indicates that the output waveform of signal A
out(t) would be approximately the reciprocal of the incident signal waveform A
in(t):
$$\begin{align}{A}_\mathrm{out}(t)\approx \frac{a}{A_{\mathrm{in}}(t)},\end{align}$$
where the coefficient a represents the amplitude gain of the OPA. We define this regime (L v < L < 2L p) characterized by such a reciprocal-type transfer function as full-back-conversion.
For a sinusoidal AM seed signal, the spectral counterpart of such a reciprocal-type transfer function is the generation and phase locking of multiple sidebands. Figure 2(b) depicts the amplitude evolution of each order sideband during the whole amplification course. The nth-order sideband refers to the frequency line that has a frequency interval of nΩ with respect to the signal frequency line. The amplitude has been normalized to that of the center frequency line. At the beginning with L < L p, there only exists the first-order sidebands (n = ±1) with a constant amplitude. This regime just corresponds to the amplification regime of conventional OPAs, where back-conversion does not occur. This explains why OPAs have never been used for sideband generation before our work.
Then at L = L p when the modulation peaks of the signal turn into back-conversion, the initial pair of sidebands declines, while the second-order sidebands (n = ±2) arise. Afterwards, higher-order sidebands gradually arise and quickly grow. We note that in the regime of full-back-conversion (L v < L < 2L p), both the amount and the amplitude of the sidebands reach the maximum. Although it has been long recognized that the temporal shape of the signal changes significantly upon back-conversion, this is the first time that the back-conversion effect is deliberately exploited for sideband generation.
In general, an OPA experiences the regimes of small-signal amplification, saturated amplification, back-conversion and full-back-conversion in sequence with the increase of crystal length. Figure 3 summarizes the spectral characteristics of the pump, signal and idler in these four regimes, which demonstrates how the multiple sidebands are induced and how the phase of all the induced sidebands evolves into an arithmetic sequence. Essentially, the interacting wave naturally experiences a phase shift of π or –π during its annihilation or creation in parametric processes[ Reference Ian, Matousek, Geoffrey and Osvay 25 ]. In the small-signal amplification regime (Figure 3(a)), the pump keeps a single frequency line with an initial phase of φ p = 0, while the three frequency lines contained by the sinusoidal AM seed signal also have an equal phase of φ s = 0. They induce an idler wave that spontaneously chooses an initial phase that satisfies φ i = φ p − φ s − π/2 to optimize signal amplification[ Reference Ma, Wang, Yuan, Xie and Qian 26 ]. So, initially the idler wave has three frequency lines with an equal phase of φ i = −π/2.
(a) The amplitude (vertical lines) and phase (red circles) of each sideband for the pump, idler and signal calculated at various crystal lengths of (a) L = 0, (b) L = L p = 12.8 mm, (c) L = 14.5 mm and (d) L = 21.5 mm. The right-hand column presents the corresponding waveforms of the signal (blue solid line), pump (black solid line) and idler (green dashed line).
Then in the regime of saturated amplification (Figure 3(b)), pump depletion becomes significant. Through the pump depletion, the signal laser imprints its sinusoidal amplitude modulation onto the pump waveform. As a result, the pump acquires a pair of sidebands. The new production of this pair of sidebands is naturally accompanied by a phase shift of ±π with respect to the initial pump phase. Afterwards, the parametric wave-mixing between the +1st (−1st) sideband of pump and the −1st (+1st) sideband of idler generates the +2nd (−2nd) sideband of signal. This pair of newly induced signal sidebands also spontaneously chooses an optimum phase that satisfies φ s = φ p − φ i − π/2. Hence, the phase of ±2nd sidebands in the signal exhibits a phase shift of ±π with respect to the initial ±1st sidebands. The presence of ±2nd sidebands in the signal wave then induces the production of ±2nd sidebands in the idler wave. After that, the OPA falls into the back-conversion regime (Figure 3(c)), where laser energy flows back from the signal and idler to the pump. Thus, the amplitude of the signal and idler declines, while the amplitude of the pump reverses to increasing. Nevertheless, the number of sidebands in the pump, signal and idler further increases due to further parametric mixing of multiple frequency lines. The regime of back-conversion leads to the nonlinear production of all the sidebands. In particular, in Figure 3(c) the ±1st sidebands bounce into reproduction after an entire back-conversion, and this reproduction is accompanied by an extra phase shift of ±π. As a result, the ±1st sidebands of the signal now have the same phase as the ±2nd sidebands.
Finally, the full-back-conversion regime is characterized by the phenomena that the number of signal sidebands reaches the maximum, and all the sidebands bounce into reproduction after experiencing an entire back-conversion. On the one hand, since the reproduction of each sideband is accompanied by a phase shift of ±π, the phase of all the sidebands constitutes an arithmetic sequence in this regime (Figure 3(d)). The temporal counterpart of such a frequency comb can be thus qualitatively evaluated as follows:
$$\begin{align}E(t)&={E}_0\exp \left(i{\omega}_0t\right)\sum \limits_{n=-N}^N\exp \left[ in\ \left(\pi +\Omega t\right)\right]\nonumber\\ & ={E}_0\exp \left(i{\omega}_0t\right)\frac{\cos \left(\frac{2N+1}{2}\Omega t\right)}{\cos \left(\frac{\Omega t}{2}\right)},\end{align}$$
where ω 0 is the center frequency of signal and 2N refers to the number of sidebands. This result signifies that an ultrashort pulse train has been generated. On the other hand, since all the sidebands have experienced an entire back-conversion, almost all the energy flows back to the pump, such that the pump depletion becomes negligible and the pump almost recovers to a single frequency line, just as in the small-signal amplification regime. In the right-hand column of Figure 3(d), we present the temporal waveform of the output pump, idler and signal in this regime, where the amplitude modulation on the pump laser (black line) becomes negligible and the output signal waveform exhibits an ultrashort pulse train. Except for the signal wave, an idler wave with the same number of sidebands is also generated.
3 Characterization of the ultrashort pulse train
In the full-back-conversion regime, numerical simulations show that the amplitude of the output signal is inversely proportional to the incident amplitude (Figure 4(a)). Consequently, the output signal waveform A out(t) fits well with the reciprocal of the incident signal waveform. With such a transfer function, a sinusoidal AM seed signal single pulse with a temporal amplitude as given by
$$\begin{align}{A}_\mathrm{in}(t)=\frac{A_\mathrm{p}+{A}_\mathrm{v}}{2}+\frac{A_\mathrm{p}-{A}_\mathrm{v}}{2}\sin \left(\Omega t-\frac{\pi }{2}\right)\end{align}$$
evolves into the following:
$$\begin{align}{A}_\mathrm{out}(t)=\frac{a}{\frac{A_\mathrm{p}+{A}_\mathrm{v}}{2}+\frac{A_\mathrm{p}-{A}_\mathrm{v}}{2}\sin \left(\Omega t-\frac{\pi }{2}\right)},\end{align}$$
(a) The output signal amplitude A out versus incident signal amplitude A in (blue), which agrees well with a reciprocal-type transfer function (red). The inset plots the incident (black) and output signal waveform calculated by numerical simulation (blue) and Equation (5) (red). (b) The spectrum of the output signal (blue) and the fitting based on Equation (10). (c) The number of sidebands (with the relative amplitude ≥0.1) and the temporal duration of the output signal against the change of ER. (d) Stability of the output pulse duration and temporal contrast against the change of crystal length.
where the coefficient a links with the amplitude of the output signal, and is related with the saturated gain provided by the χ(2) parametric process. With a saturated gain of g, then the coefficient can be simply expressed by a = g(A v)2. In Equation (4), t = 0 corresponds to a valley of the incident signal, while in Equation (5), the point of t = 0 becomes a modulation peak. Around t = 0, Equation (5) can be approximated into the following:
$$\begin{align}{A}_\mathrm{out}(t)\approx \frac{4a/{A}_\mathrm{p}}{{\left(\Omega t\right)}^2+4{A}_\mathrm{v}/{A}_\mathrm{p}}.\end{align}$$
Note that such a waveform is highly coincident with that of a Lorentz-shaped pulse, as follows:
$$\begin{align}{A}_\mathrm{LZ}(t)=\frac{1}{\pi}\cdot \frac{\Gamma}{t^2+{\Gamma}^2}.\end{align}$$
Thereby, the temporal duration of the output pulse is dominated by the parameter Γ, which in our case is equal to the following:
$$\begin{align}\Gamma =\sqrt{\frac{4{A}_\mathrm{v}}{\Omega^2{A}_\mathrm{p}}}=\frac{2}{\Omega \sqrt[4]{\mathrm{ER}}}.\end{align}$$
The pulse duration at half magnitude can thus be solved as follows:
$$\begin{align}T=2\sqrt{\sqrt{2}-1}\Gamma \approx 1.29\Gamma.\end{align}$$
The output pulse duration is proportional to the parameter Γ, which is inversely proportional to the modulation frequency Ω as well as the fourth root of the ER of the incident sinusoidal AM signal (
${A}_\mathrm{p}/{A}_\mathrm{v}=\sqrt{\mathrm{ER}}$
). The limit of the output pulse duration can be estimated using Equations (8) and (9). For such a Lorentz-shaped output pulse, the spectrum can be approximately given by the following:
$$\begin{align}{a}_\mathrm{LZ}\left(\omega \right)={e}^{-\Gamma \left|\omega \right|}.\end{align}$$
Figure 4(b) shows the spectral amplitude of the output pulse, wherein the blue solid line presents the result obtained for numerical simulation, while the red dashed line depicts the approximate solution calculated based on Equation (10). The spectrum exhibits exponential decay in the leading and trailing wings. The good agreement between the numerical simulation results with Equations (7) and (10) verifies that an OPA operating in the full-back-conversion regime can translate a sinusoidal AM laser into a train of Lorentz-shaped pulses.
A sinusoidal AM seed signal with higher ER induces a train of pulses with shorter duration. As shown in Figure 4(c), an ER of 30 dB leads to the generation of 12 sidebands, while an ER of 50 dB leads to 36 sidebands in our simulated case. The former corresponds to a temporal pulse duration of 1.8 ps, while the latter corresponds to 0.6 ps. The temporal duration and the contrast of the output pulses are stable within the whole regime of full-back-conversion (i.e., the crystal length range of 19–25 mm), as indicated by Figure 4(d). In addition, the proposed scheme not only transforms a sinusoidal AM seed signal into a picosecond pulse train, but also amplifies the signal in amplitude. In our case, the output pulse amplitude around t = 0 has a saturated gain of approximately 104. This means that the output pulse intensity is approximately 105 times stronger than the peak intensity of the AM seed signal.
4 Practical consideration
OPAs inherently suffer from the PSF noise[ Reference Salerno, Minardi, Trull, Varanavicius, Tamosauskas, Valiulis, Dubietis, Caironi, Trillo, Piskarskas and Trapani 27 ]. Next we identify the effect of PSF on the generation of the picosecond pulse train. A zero-mean stochastic phasor with a uncorrelated Gaussian distribution is introduced into the initial signal wave to mimic the spontaneous parametric down-conversion noise[ Reference Moses, Huang, Hong, Mücke, Falcão-Filho, Benedick, Ilday, Dergachev, Bolger, Eggleton and Kärtner 28 , Reference Wang, Ma, Wang, Yuan, Xie and Qian 29 ]. The initial energy of the noise field is assumed to be 40 aJ, as given in Ref. [Reference Moses, Huang, Hong, Mücke, Falcão-Filho, Benedick, Ilday, Dergachev, Bolger, Eggleton and Kärtner28]. The simulation results show that the presence of PSF does imprint some stochastic amplitude noise onto the output pulse train (Figure 5(a)). However, it has a negligible influence on both the temporal shape and duration of the output pulses. Given that the PSF noise has a bandwidth much wider than the picosecond pulse train, it can be feasibly removed by a bandpass filter. The red lines in Figures 5(a) and 5(b) depict the temporal and spectral amplitude of the output picosecond pulse after bandpass filtering, respectively, which indicates that the influence of PSF has been overcome.
(a) Temporal waveform and (b) power spectral density of the output pulse train calculated in the presence of PSF without (blue) and with bandpass filtering (red), respectively. Temporal waveform of the output pulse train calculated for (c) GVM si = 0 (black), 90 fs/mm (blue), 500 fs/mm (red) and (d) GVM sp = 0 (black), 800 fs/mm (blue), 1200 fs/mm (red). Other simulation parameters are set the same as in Figures 3(d) and 4(a).
Finally, we study the influence of the medium dispersion. In the context of generating a picosecond pulse train (corresponding to a spectral bandwidth of less than 1 THz), only the first-order dispersion, that is, the group-velocity mismatch (GVM), needs to be considered. In general, the GVM between the interacting waves can cause a temporal shift of the output pulse train. This temporal shift will degrade the A p/A v ratio in Equation (6), which thus has the probability to degrade the temporal duration and contrast of the output picosecond pulse train. For the GVM between the signal and idler wave (GVM si), numerical simulations reveal that as long as the overall temporal shift caused by GVM si is less than the output pulse duration, its influence is negligible. The above simulations, under the assumption of zero GVM, result in an output pulse duration of 1.8 ps (Figure 4(a)). Given that a crystal length of L ≥ 20 mm is required for full-back-conversion, the critical value for GVM si is approximately 90 fs/mm. Figure 5(c) plots the output pulse train calculated with GVM si = 90 fs/mm, which exhibits only a temporal shift relative to the ideal condition with GVM si = 0. The duration and contrast of each pulse are nearly unchanged. When we purposely increase GVM si to 500 fs/mm, the pulse duration increases from 1.8 to 3.3 ps, and the pulse contrast dramatically degrades from 30 to 13.5 dB. Practically, the GVM si in PPLN crystal is only 20 fs/mm, which is much less than the critical value of 90 fs/mm, indicating that the influence of GVM si is negligible.
Since the pump laser is initially a quasi-continuous-wave, the effect of the GVM between the pump and signal (GVM sp) is much less important compared with GVM si. In our simulated case, GVM sp (= 800 fs/mm) only causes a very small temporal shift of the output pulse train, as shown in Figure 5(d). Even when we increase GVM sp to 1200 fs/mm purposely, the duration of each pulse does not change, and only the pulse contrast falls into degradation.
The above practical considerations show that the production of an ultrashort pulse train from parametric wave-mixing prefers a sinusoidal AM seed signal with a high ER and a nonlinear medium with small dispersion GVM si and high nonlinear coefficient d eff. A high d eff is desirable because large nonlinear length (proportional to d eff as well as the crystal length L) is indispensable to transfer an AM signal of high ER into the full-back-conversion regime. If a nonlinear medium with small d eff is used, a large crystal length becomes necessary to reach full-back-conversion, which increases the PSF as well as the temporal walk off between the signal and idler, thereby degrading the temporal contrast of the output ultrashort pulse train.
5 Conclusion
In conclusion, we propose a χ(2)-based optical modulator that provides a reciprocal-type transfer function, and further demonstrate that such an optical modulator can directly transfer a sinusoidal AM laser into a train of Lorentz-shaped picosecond pulses, without the need for optical resonators. Being different from conventional χ(2) parametric processes, the back-conversion effect that is carefully avoided in previous applications is exploited in our scheme. It is the strong nonlinearity inherent to back-conversion that induces multiple sideband generation and finally enables a reciprocal-type transfer function. Meanwhile, the inherent phase shift of π that accompanies photon annihilation or creation in parametric processes plays an important role in driving all the induced sidebands into phase locking.
Compared to traditional mode-locking techniques, our proposed scheme for producing ultrashort pulse train does not require optical resonators. Thus, it does not require complex alignment and promises a higher pulse repetition rate. The repetition rate of the output picosecond pulse train is exactly equal to the modulation frequency of the AM seed signal. It has been reported that a sinusoidal AM signal with a modulation frequency of THz can be produced by the optical beat between two narrow frequency lines[ Reference Schimpf, Olgun, Kalaydzhyan, Hua, Matlis and Kärtner 30 ]. The combination of such a THz modulation and our proposed scheme promises the generation of an ultrashort pulse train with a repetition rate as high as THz, which is impossible by mode-locked laser techniques so far. Another difference is the temporal and spectral characteristics of the output pulses. The pulses produced by our proposed scheme are Lorentz-shaped in the time domain, and the frequency combs contained in the spectrum exhibit exponential decay in two wings. The phase of all the frequency combs constitutes an arithmetic sequence with a phase shift of π between adjacent combs.
Such a high-speed ultrashort pulse train has implications for the efficient generation of multi-cycle THz waves[ Reference Ravi, Schimpf and Kärtner 31 ]. Previously, THz modulations were produced by optical beating among multiple frequency lines or chirped pulses with various delays[ Reference Stummer, Flöry, Krizsán, Polónyi, Kaksis, Pugžlys, Hebling, Fülöp and Baltuška 32 – Reference Chen, Zhou, Werley and Nelson 34 ], which were not so stable and difficult to adjust. By comparison, our scheme only requires one single-stage OPA, and thus is much more compact, stable and tunable. In addition, the generation of a picosecond pulse train at signal wavelength is naturally accompanied by the production of another picosecond pulse train at idler wavelength. This implies the potential to directly produce a powerful picosecond pulse train at THz repetition rate in the mid-infrared spectral range.
Acknowledgement
This work was supported by the National Natural Science Foundation of China (Nos. 61727820, 61905142, 61975120, and 91850203).
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