Broadband time-reversal of optical pulses using a switchable photonic-crystal mirror

Recently, Chumak et al. have demonstrated experimentally the time-reversal of microwave spin pulses based on non-adiabatically tuning the wave speed in a spatially-periodic manner. Here, we solve the associated wave equations analytically, and give an explicit formula for the reversal efficiency. We then discuss the implementation for short optical electromagnetic pulses and show that the new scheme may lead to their accurate time-reversal with efficiency higher than before.

Time-reversal is one of the most spectacular and useful wave phenomena. A time-reversed pulse evolves as if time runs backward, thus eliminating any distortions or scattering that occurred at earlier times. This enables light detection, imaging and focusing through complex media [2,3] with applications in diverse fields such as medical ultrasound [2], communication systems and adaptive optics [4], superlensing [5], ultrafast plasmonics [6], biological and THz imaging [7], spintronics [8] and quantum information and computing [9].
For low frequency waves (e.g., in acoustics, microwave spin/electromagnetic waves etc.), time-reversal can be accomplished by electronic sampling, recording, and playing back [2]. This is possible since in this frequency range, the pulse oscillates on a scale slower than electronic sampling speed. On the other hand, for high frequency waves, specifically, for optical electromagnetic waves, the pulse oscillations (and even the pulse envelope itself for sufficiently short pulses) are too short to be sampled properly by even the fastest electronic detector.
The standard solution in the optical regime is to use nonlinear processes such as Three-Wave or Four-Wave Mixing (3WM or 4WM, respectively), see e.g., [4,11,12,13]. However, while such techniques have been demonstrated experimentally, they usually suffer from one or several disadvantages. In particular, they require fairly high intensities, thus, limiting onchip integration; almost all existing schemes are narrowband whereas the schemes which are applicable to relatively short pulses are in general complex, requiring complicated setups and sometimes even cryogenic temperatures. Finally, some schemes may be difficult to apply to 2and 3-dimensional systems.
Recent suggestions to overcome some of these limitations involved dynamically-tuned optical periodic structures, known as photonic crystals (PhCs) [15,16]. However, despite being very efficient, the structures and/or modulations required for these schemes were quite challenging to realize; in addition, these schemes allow for reversal of only relatively narrow pulses. However, these obstacles were recently lifted in a study by Chumak et al. [1]. In particular, it was shown in [1] that a pulse propagating in a homogeneous material can be time-reversed if the material is subject to a spatially-periodic, time-localized non-adiabatic modulation. This scheme is closely related to other non-adiabatic optical pumping based schemes which were studied theoretically earlier in slab waveguides [10,14], atomic vapours [17] and zero-gap photoniccrystals [18,19].
In this article, we study the time-reversal scheme of [1] theoretically and compare it to previous non-adiabatic modulation-based schemes; we focus on time-reversal of ultrashort optical pulses, which as noted above, still has not been demonstrated experimentally. We first give a simple heuristic explanation of the dynamically-tuned PhC-based schemes [1,18,19] showing that the reversal originates from switching-on a bulk PhC mirror (Section 1). Then, we provide a detailed analytical study of the reversal process in [1], derive a simple explicit formula for the reversal efficiency in the weak-coupling limit and compare it with existing techniques (Section 2). We then briefly discuss the implementation for optical electromagnetic pulses (Section 3).

Principles of time-reversal using a switchable mirror
In order to understand the reversal schemes of [1,18,19], it is beneficial to adopt a somewhat heuristic interpretation. Recall that when a pulse is reflected by a (standard) mirror, its spatial components change their propagation direction at different times, i.e., the leading edge first and trailing edge last. Thus, the pulse effectively undergoes a U-turn, i.e., the leading edge remains the leading edge etc.. Now, imagine that one could change of direction of the pulse propagation at all points in space and at the same time. Then, obviously, the leading edge will become the trailing edge, and vice versa, i.e., the pulse is (time-) reversed.
In order to perform such an extreme manipulation, one needs to abruptly reduce the transmissivity of the medium, preferably to zero, everywhere is space and for a spectral band as wide as possible. Possibly the simplest way to do that would be to open a frequency bandgap by periodically modulating the material properties. Heuristically, when the bandgap is turned on, the wave cannot propagate in any direction. Instead, the forward waves are then repeatedly converted to backward waves, then back to forward waves and vice versa. If one re-establishes the transmissivity once most of the energy of the forward wave has been converted to a backward wave, then a time-reversed pulse is released backwards. In a sense, this procedure transforms a perfectly transmitting medium into a "volume" mirror. Accordingly, in what follows we refer to these schems as switchable mirror (SM) -based reversal schemes.
This heuristic explanation clarifies why the zero-gap-based switchable-mirror (ZGSM) is equivalent to a homogeneous-medium-based switchable-mirror (HSM). Indeed, unlike a finitegap system, in both structures all the incident light is perfectly admitted. In addition, in both structures a gap is opened due to the modulation (see [1,19]). It is also implied by the heuristic explanation (and later proved analytically in Section 2), that in both ZGSM and HSM, although the wave-front is reversed, it is not conjugated. Thus, the scheme can lead to perfect timereversal only if it is complemented by a consequent step of phase-conjugation, e.g., via nearlydegenerate 4WM [18,19]. As shown in Section 2, this may also be beneficial in order to make the scheme more efficient.
The advantage of the SM-based schemes is the ability to reverse pulses of almost unlimited wide spectrum. Indeed, the only limitation is the shortness of the modulation. Also, as noted in [1,18,19], the new reversal schemes, which require only a periodic modulation rather than complex optics-specific concepts, open the way for time-reversal in many other wave systems for which time-reversal was not accessible before, such as atomic physics [17], quantum computing [9] etc.. Importantly, the HSM has several advantages over the ZGSM. First, the former is obviously simpler as essentially no fabrication is required; its performance is also practically insensitive to the modulation spatial pattern. Second, our analysis (Eq. (16) below) shows that the reversal effeciency of the in a HSM is about an order of magnitude higher than in a ZGSM. Third, while the frequency conversion performed in a ZGSM is purely vertical [18,19], the frequency conversion in a HSM involves also a change in the sign of the carrier wavevector, i.e., the dynamic grating provides the momentum to allow a horizontal transition between positive to negative momentum [1]. As a result, the out-coupling of pulses from the HSM is not plagued by reflections at the boundaries, as may happen in a ZGSM. A final advantage of the HSM is that by choosing the proper modulation pattern, the reversal can be performed for any angle of incidence, for plane-waves as well as for beams, for high dimensional gratings or waveguide structures as well as for any incident carrier frequency.

Analysis
In this Section we derive the coupled envelope equations and solve them analytically in the weak-coupling limit. Since the former step is very similar to the derivations in [20], and latter step is almost identical to the procedure detailed in [18,19], here, the derivation and solution are given quite briefly.
Consider an electromagnetic plane-wave pulse propagating along the x-direction in a homogeneous medium which is time-modulated in the following manner Here, n 0 is the average refractive index, the modulation is spatially periodic, i.e., and time-localized around t 0 with max[m(t − t 0 )] = m(t 0 ) = 1, i.e., the modulation essentially turns on a periodic grating perpendicular to the direction of propagation of the pulse. In this case, the Maxwell equations reduce to the 1D wave equation In order to solve Eq. (3), we follow the derivation given in [20], used previously to study the propagation of optical pulses in a photonic crystal with a cubic (Kerr) nonlinear response 1 . We assume the field can be written as where E ± represent the Slowly-Varying Envelopes (SVEs) of the forward and backward field compoenets, respectively; ω 0 = ck 0 , k 0 = 2πn 0 /λ v and n 0 are the carrier frequency, wavevector and refractive index of the medium, respectively, with λ v being the vacuum wavelength. Substituting the ansatz (4) into Eq. (3), neglecting the c.c. terms and the second order derivative terms, and removing the factor e −iω 0 t gives The spatial modulation ε m (x) couples the forward and backward field components. When k 0 is close to the first bandgap, i.e., when k 0 = k (g) + δ k (with k (g) ≡ π/d or equivalently, λ (g) v = 2n 0 d), the j = ±1 components of the grating are close to the phase mismatch between the forward and backward field components, so that the coupling becomes most efficient. Following [20], we now expand the spatial part of the modulation as a Fourier series as follows