Frequency Down-Conversion of Optical Pulse to the Far Infrared and THz Frequency Ranges Due to the Cascading Process in a Medium with a Quadratic Nonlinear Response

Abstract

Difference-frequency generation is a well-known method of obtaining IR and THz radiation. It has many practical applications, such as sensing, optical metrology, diagnostics, detection and identification of substances, etc. One of the generation methods is based on the three-wave interaction in a medium with second-order nonlinear susceptibility. In this study, we investigated a special case of the frequency down-conversion into IR and THz ranges of the frequencies: the frequencies of interacting waves were multiple. We analyzed theoretically two cases of three-wave interactions: amplification of the infrared (or THz) radiation (incident weak intensity of a wave at this frequency) and a wave generation with the difference-frequency (incident zero-value intensity at this frequency). The amplification efficiency could achieve 75% and the maximal frequency conversion efficiency is about 25%. The computer simulation results made for the femtosecond pulse interaction in a crystal with the wavelength 4, 10, and 24 μm demonstrates applicability of such a scheme for the frequency down-conversion. This scheme of the THz radiation generation is a perspective tool for its application in the screening system for the detection and identification of substances.

1. Introduction

Infrared optics and THz optics have various practical applications, including spectroscopy [1,2], optical metrology [3], material measurements [4], sensing [5], diagnostics, detection, identification of substances, etc. One of the possible ways to obtain laser radiation in these ranges of the frequencies is via a frequency down-conversion process, due to the difference frequency’s wave generation in a medium with a quadratic nonlinear response.

The difference frequency’s wave generation, whose frequency belonging to an infrared frequencies range, has attracted the attention of many researchers. Below, we mention some of them. In [6], the femtosecond pulses with tunable wavelengths belonging to the interval (3.2–4.8 μm), and possessing a maximal average power of about 1.1 mW, were generated in the MgO:LiNbO₃ crystal. In [7], a tunable source of the mid-infrared CW radiation with a maximal power of 51 mW at a wavelength ${\lambda }_1=6543$ nm was created based on the difference frequency’s wave generation in a GaAs crystal. Optical frequency combs with wavelengths belonging to their intervals (2.8–3.5 μm) were generated in MgO:PPLN crystal using the difference frequency’s wave generation [8]; a similar result was also obtained in GaSe crystal with the frequency combs generation, in the wavelength range 3–10 μm [9].

Frequency down-conversion also consists of using the optical parametric oscillation process. Thus, in [10], by using this tool, a conversion efficiency of 34% was achieved with the average output power of 7.7 W at the power of the incident pump pulse equal to 23 W. The IR radiation at a wavelength 7 μm with an energy of 0.71 mJ was obtained with a 7.8% quantum conversion efficiency in BaGa₄Se₇ crystal [11]. Tunable IR radiation generation belonging to the wavelength range 4.4–5.7 μm, with a maximal output energy of 13.1 μJ, was achieved in [12], using La₃Ga_5.5Nb_0.5O₁₄ crystal. A review of the frequency down-conversion processes in non-oxide media can be found in [13].

A THz radiation source using difference-frequency generation was also obtained in many nonlinear media. For example, a THz pulse with the wavelength in the range of 290–140 μm was realized in a LiNbO₃ crystal [14]. The periodically-poled LiNbO₃ crystal was used in [15], the frequency range was 1.5–1.8 THz; a maximal power was equal to 0.1 mW); and in [16], the wavelength range was 190–210 μm and 457–507 μm; the maximal energies were equal to 0.37 and 0.057 pJ, respectively; in [17], the authors explored the realization of a generation scheme of the difference-frequency equal to 0.5 THz with a conversion efficiency of 30%.

It should be noted that, in a series of studies, i.e., [18,19,20,21] and the corresponding references listed in those papers, the THz radiation with a wavelength range of 66.5 μm, 5664 μm was obtained in crystals GaSe, ZnGeP₂ GaP based on difference frequency’s wave generation with conversion efficiency equal to 0.1%.

Crystal ZnTe is often used for frequency down-conversion to obtain a THz radiation. We can note, for example, the following papers: [22], where pulse 1 THz was obtained as 365 and 364 THz frequency differences and with a 0.6% conversion efficiency. In Reference [23], the authors demonstrated the possibility of pulse generation with tunable frequency, in the range of 0.3–2.5 THz, and power up to 1 μW based on difference-frequency generation involving interactions of picosecond pulses, with intensity at 2.58 × 10⁸ W/cm² generated with 1.5% conversion efficiency.

In another THz pulse source with tunable frequency, the frequency range was 0.3–19.6 THz, with energy at 870 nJ, and was obtained in the DAST crystal lit by an incident pulse with a power density of 247 MW/cm² [24]. Using a GaSe crystal with a length of 8 mm and a down-conversion frequency process, a source of the tunable frequency, belonging to a frequency range of 0.21–3 THz, and conversion efficiency equal 0.00168%, was created [25]. A review of the sources of the THz radiation based on the frequency down-conversion process is presented in [26]. In turn, a review of quantum cascade lasers using the the difference-frequency generation process for obtaining THz radiation is found in [27]. It should be noted that a process of the difference-frequency generation was also used for developing THz CW spectrometers based on lithium niobate channel-waveguides [28], which is important regarding the problem of substance detection and identification.

A crystal AgGaS₂ is widely used for IR radiation generation [29,30,31,32,33]. IR radiation generation with wavelength intervals at 3.9 μm and 9.4 μm, at incident pulse durations in picosecond ranges, was discussed in [29]. The achieved conversion efficiency of the energy transform was a few percent for the incident pulse energy of 10 mJ. The difference-frequency generation was chosen as a base of the IR spectrometer [30]. The pulses possessing the energy (10 μJ) and duration (50 ns), and wavelength intervals at 3–12 μm, were obtained in [31]. The femtosecond pulse interaction scheme used for obtaining pulses with a tunable frequency in the mid-infrared range and output energy, equaling several mJs, was discussed in [32]. The source of pulses, constructed using the difference-frequency generation with the efficiency 0.6%, with tunable wavelength intervals at 5–12 μm, and a duration 8 ns, was presented in [33].

In past years, the frequency up-conversion in the tellurium chains have been widely discussed (see, for example, [34]); thus, one may expect the frequency down-conversion process in this crystal will be effective. The tellurium crystal has a big transmittance range in the infrared range of the wavelengths (at least until 24 μm, according to [35]), and a large second-order susceptibility [36]. The frequency down-conversion to the range of the mid-infrared frequencies with a peak power of 100 μW, achieved in tellurium crystal with a length 11 μm, is presented in [37].

In the current study, we propose a new approach for the frequency down-conversion to infrared (or even THz) range using the difference-frequency generation at wave interactions with multiple frequencies ω (low-frequency wave, LFW), 2ω (intermediate frequency wave, IFW), 3ω (high-frequency wave, HFW), in the case of large phase-mismatching between two interacting waves. To our knowledge, such a scheme, regarding the frequency down-conversion, has not been discussed in previous literature. We present the computer simulation results for the frequency down-conversion of femtosecond pulses, with duration equal to 100 fs for the pulses with corresponding wavelengths, 4 μm (75 THz), 10 μm (50 THz; belongs to the infrared frequencies range), and 24 μm (12.5 THz; belongs to the THz frequencies range), if the LFW and HFW interact in the phase-matched mode and the phase mismatching between IFW and LFW is large enough. Therefore, it allowed us to apply the multi-scale method to derive the modified set of equations and to solve those equations analytically in the long pulse duration approximation framework and plane wave approximation, but without using the energy non-depletion approximation of HFW.

The computer simulation is provided for two well-known crystals—AgGaS₂ and tellurium. Our calculations, based on the results of the Sellmeier equations, taken from study [38], show that it is possible to achieve phase matching between LFW and HFW in this crystal at the LFW wavelength, up to 10 μm in the crystal AgGaS₂. Thus, we use this crystal’s data for the frequency down-conversion into the radiation possessing wavelength equal to 4 μm and 10 μm, and the tellurium crystal data [39] for the frequency down-conversion to wavelength 24 μm.

Our paper is organized as follows. We begin with the set of nonlinear Schrödinger equations accounting for the group velocity dispersion (GVD) of the laser pulses. Then, based on the multi-scale method, we derive the modified set of equations and solve them without using the energy non-depletion approximation for HFW in the framework of the long pulse duration approximation. This solution demonstrates that the effective energy conversion of HFW to LFW is possible, even if the incident IFW’s intensity is small.

The latter part of our study contains computer simulation results, showing how GVD influences energy conversion efficiency. That section is divided into two parts: investigation of the amplification process (small incident LFW’s intensity) and the generation process (incident LFW’s intensity is equal to zero). In both cases, we demonstrate that a highly-effective frequency down-conversion process occurs under certain conditions.

2. Problem Statement

The three-wave interaction process with multiple frequencies in a medium with quadratic nonlinear responses can be described by the set of nonlinear Schrödinger equations [40]:

$$\begin{array}{c}\frac{\partial A_1}{\partial z}+i{D}_1\frac{{\partial }^2{A}_1}{\partial t^2}+i\left({\gamma }_{12}{A}_1^{*}{A}_2{e}^{-i{\Delta }_{21}kz}+{\gamma }_{23}{A}_2^{*}{A}_3{e}^{-i({\Delta }_{31}k-{\Delta }_{21}k)z}\right)=0,\hfill \\ \frac{\partial A_2}{\partial z}+{\nu }_{21}\frac{\partial A_2}{\partial t}+i{D}_2\frac{{\partial }^2{A}_2}{\partial t^2}+i\left({\gamma }_{11}{A}_1^2{e}^{i{\Delta }_{21}kz}+2{\gamma }_{13}{A}_1^{*}{A}_3{e}^{-i({\Delta }_{31}k-{\Delta }_{21}k)z}\right)=0,\hfill \\ \frac{\partial A_3}{\partial z}+{\nu }_{31}\frac{\partial A_3}{\partial t}+i{D}_3\frac{{\partial }^2{A}_3}{\partial t^2}+3i{\gamma }_{21}{A}_1{A}_2{e}^{i({\Delta }_{31}k-{\Delta }_{21}k)z}=0,0<z\le L_z.0<t<L_t.\hfill \end{array}$$

(1)

The initial condition and boundary conditions (BCs) are the following:

$$\begin{array}{c}{A}_1(0,t)=A_{10}\left(t\right),A_2(0,t)=A_{20}\left(t\right),A_3(0,t)=A_{30}\left(t\right),t\in [0,L_t],\hfill \\ A_1(z,0)=A_2(z,0)=A_3(z,0)=A_1(z,L_t)=A_2(z,L_t)=A_3(z,L_t)=0,z\in [0,L_z],\hfill \end{array}$$

(2)

which correspond to the absence of the laser radiation of all optical waves out of a certain time interval. Here, $A_j$ are dimensionless complex amplitudes of LFW, IFW, and HFW. Coefficients ${\gamma }_{jk}$—of nonlinear coupling of interacting waves—characterize a second-order nonlinear response at the corresponding frequencies. Below, for simplicity, we omit a dependence of this coefficient on the optical frequency. Therefore, these coefficients are equal to the same value: ${\gamma }_{jk}=\gamma$. We emphasize that this is not a strong restriction for our analysis. Parameters ${\Delta }_{21}k$ and ${\Delta }_{31}k$ denote dimensionless phases mismatching between IFW and LFW, and HFW and LFW, respectively. Coefficients ${\nu }_{21}$ and ${\nu }_{31}$ are dimensionless mismatching of the group velocities between pulses of IFW and LFW, and HFW and LFW, respectively. Parameters $D_1,D_2$ and $D_3$ are dimensionless coefficients of the second order dispersion (SOD) at the corresponding frequencies, characterizing GVD of the propagating pulses. t and z are dimensionless time and space coordinates, correspondingly.

Let us note that the diffraction is not taken into account in Equation (1). This is valid if the radii of the incident beams are large enough to satisfy the following conditions: the diffraction length is greater than the crystal’s length and the nonlinear length, which is defined by the incident beam’s maximal intensity. Such conditions often occur in physical experiments (see, for example, [41,42,43]). Writing Equation (1), we neglected the cubic nonlinear response of a crystal. It can be done if the maximal intensity of the incident pulse is less than the certain value, depending on the used crystal [40].

The dimensionless variables and parameters are expressed through the physical ones as follows:

$$\begin{array}{c}{\nu }_{j1}=\left(\frac{\partial \overline{k}}{\partial \overline{\omega }}{{|}_{{\overline{\omega }}_j}-\frac{\partial \overline{k}}{\partial \overline{\omega }}|}_{{\overline{\omega }}_1}\right)\frac{Z_n}{{\tau }_p},j=2,3,D_j=-\frac{1}{2}\frac{{\partial }^2\overline{k}}{\partial {\overline{\omega }}^2}{|}_{{\overline{\omega }}_j}\frac{Z_n}{{\tau }_p^2},A_j=\frac{{\overline{A}}_J}{A_0},j=1,2,3,\hfill \\ \gamma =\frac{2\pi {\chi }^{\left(2\right)}{\overline{k}}_1{A}_{01}}{n^2}{Z}_n,{\Delta }_{21}k={\Delta }_{21}\overline{k}{Z}_n,{\Delta }_{31}k={\Delta }_{31}\overline{k}{Z}_n.\hfill \end{array}$$

(3)

where ${\tau }_p$ is the incident pulse duration of the LFW (${\overline{\omega }}_1=\overline{\omega }$), which is chosen to be equal to 100 fs, if we do not specify otherwise. Time coordinates are measured in ${\tau }_p$. Parameter $Z_n$ is a normalization length chosen equal 1 mm. The propagation distance of the optical pulse is measured in this units. Coefficients ${\chi }^{\left(2\right)}({\overline{\omega }}_j,{\overline{\omega }}_l)$ are the quadratic susceptibilities of a medium at the frequencies $\overline{{\omega }_j},\overline{{\omega }_l}$. The frequency ${\overline{\omega }}_j=j\overline{\omega }$ is associated with the wavelength ${\lambda }_j$ by the known ratio: ${\overline{\omega }}_j=2\pi c/{\lambda }_j,j=1,2,3$. Parameter ${\overline{k}}_1$ is a dimensional wave-number of the LFW. In turn, ${\Delta }_{21}\overline{k}$ and ${\Delta }_{31}\overline{k}$ are dimensional phases mismatching between the IFW or the HFW and the LFW, respectively: ${\Delta }_{j1}\overline{k}={\overline{k}}_j-j{\overline{k}}_1,j=2,3$. Parameters ${\overline{k}}_2,{\overline{k}}_3$ are the wavenumbers at the frequencies ${\overline{\omega }}_2,{\overline{\omega }}_3$, respectively. Variables ${\overline{A}}_j$ are the complex envelopes of the wave packets measured in physical units. $A_0$ is a normalization value, which is chosen as the squared root of the LFW and HFW intensities sum at their pulse centers.

In

Table 1. Characteristics of nonlinear crystal.

${\mathit{\lambda }}_1$	${\mathit{I}}_0\left({\mathbf{GW}/\mathbf{cm}}^2\right)$	$\mathit{\theta }{(}^{\circ })$	$\frac{{\mathit{d}}^2\overline{\mathit{k}}}{\mathit{d}{\overline{\mathit{\omega }}}^2}{|}_{\mathit{\omega }={\mathit{\omega }}_1}({\mathbf{m}}^{-1}$ ${\mathbf{s}}^2)$	$\frac{{\mathit{d}}^2\overline{\mathit{k}}}{\mathit{d}{\overline{\mathit{\omega }}}^2}{|}_{\mathit{\omega }={\mathit{\omega }}_2}({\mathbf{m}}^{-1}$ ${\mathbf{s}}^2)$	$\frac{{\mathit{d}}^2\overline{\mathit{k}}}{\mathit{d}{\overline{\mathit{\omega }}}^2}{|}_{\mathit{\omega }={\mathit{\omega }}_3}({\mathbf{m}}^{-1}$ ${\mathbf{s}}^2)$
4 μm (AgGaS2, [38])	6.12	49.46	4 × 10−27	2.5 × 10−25	4.34 × 10−25
10 μm (AgGaS2, [38])	20.66	79.51	−3.2 × 10−24	−1.51 × 10−24	−8.28 × 10−25
24 μm (Te, [39])	0.11	15.78	−4.36 × 10−24	1.58 × 10−24	3.08 × 10−24

, we present the physical parameters at various frequencies in a dependence of the wavelength of LFW (4, 10, and 24 μm, respectively). These values were used in the computer simulation and can be used for the arrangement of the physical experiment.

Among them, we also present the angle θ between the laser pulse propagation direction and the crystal axis, at which the phase matching between the LFW and HFW occurs (so we assume that ${\Delta }_{31}k=0$). We also present the sum incident intensity of the LFW and HFW $I_0$, at which the parameter γ equals unity. This choice is explained by our further analysis. It should be noted that the phase mismatching between the IFW and LFW is partly defined by the condition ${\Delta }_{31}k=0$. Thus, the phase matching angle θ and the phase mismatching are computed on the basis of Sellmeier equations, taken from [38,39], using the formulas that can be found, for example, in [40] (paragraph 2.3).

Below, we also neglect the group velocity mismatching: ${\nu }_{21}={\nu }_{31}=0$ to clarify the SOD influence on the frequency conversion efficiency. This imposes certain restrictions on the crystal length and the pulse durations, which should be large enough to avoid the running away from each other at the output face of the crystal. If the pulse duration is about 1 ps, then such a length can achieve a value about a few dozens of centimeters. If the pulse duration is about 100 fs, then the group velocity mismatching does not essentially influence the conversion efficiency, until ten centimeters of the optical pulse propagation distance. It only changes the pulse shapes by making them asymmetric.

3. Modified Equations Derived in the Framework of the Multi-Scale Method

3.1. Set of Modified Equations

If the phase mismatching between LFW and IFW is much larger than the nonlinear coefficient ($|{\Delta }_{21}k|>>\gamma$), we can derive the qualitative approximation of the problem (1), (2) solution using the multi-scale method:

$$\begin{array}{c}{A}_1=U+\frac{1}{{\Delta }_{21}k}\left(\gamma (U^{*}V{e}^{-i{\Delta }_{21}kz}-V^{*}W{e}^{i{\Delta }_{21}kz})+u_1\right),\hfill \\ A_2=V+\frac{1}{{\Delta }_{21}k}\left(-\gamma (U^2+2U^{*}W)e^{i{\Delta }_{21}kz}+v_1\right),\hfill \\ A_3=W+\frac{1}{{\Delta }_{21}k}\left(3\gamma UV{e}^{-i{\Delta }_{21}kz}+w_1\right),\hfill \end{array}$$

(4)

with accuracy of $O\left({\Delta }_{21}{k}^{-2}\right)$. Here, the functions U, V, W are governed by the following set of equations:

$$\begin{array}{c}\frac{\partial U}{\partial z}+i{D}_1\frac{{\partial }^{2}U}{\partial t^2}-i\tilde{\alpha }{(|U|}^{2}U+3U^{*2}W-{4U|V|}^2+{2U|W|}^2)=0,\hfill \\ \frac{\partial V}{\partial z}+{\nu }_{21}\frac{\partial V}{\partial t}+i{D}_2\frac{{\partial }^{2}V}{\partial t^2}+2i\tilde{\alpha }{(4|U|}^2-{|W|}^2)V=0,\hfill \\ \frac{\partial W}{\partial z}+{\nu }_{31}\frac{\partial W}{\partial t}+i{D}_3\frac{{\partial }^{2}W}{\partial t^2}-3i\tilde{\alpha }(U^3+{2|U|}^{2}W+{|V|}^{2}W)=0,\hfill \end{array}$$

(5)

where $\tilde{\alpha }={\gamma }^2/{\Delta }_{21}k$. The functions $u_1,v_1,w_1$ are the solutions of the following linear equations:

$$\begin{array}{c}\frac{\partial u_1}{\partial z}+i{D}_1\frac{{\partial }^2{u}_1}{\partial t^2}=0,\hfill \\ \frac{\partial v_1}{\partial z}+{\nu }_{21}\frac{\partial v_1}{\partial t}+i{D}_2\frac{{\partial }^2{v}_1}{\partial t^2}=0,\hfill \\ \frac{\partial w_1}{\partial z}+{\nu }_{31}\frac{\partial w_1}{\partial t}+i{D}_3\frac{{\partial }^2{w}_1}{\partial t^2}=0.\hfill \end{array}$$

(6)

Let us note that the derivation of these equations is made in Appendix A. The distributions for the new functions corresponding to the complex amplitudes of the incident pulses are the following:

$$\begin{array}{c}U(0,t)=A_{10}\left(t\right),V(0,t)=A_{20}\left(t\right),W(0,t)=A_{30}\left(t\right),\hfill \\ u_1(0,t)=\gamma \left(A_{20}^{*}\left(t\right)A_{30}\left(t\right)-A_{10}^{*}\left(t\right)A_{20}\left(t\right)\right),v_1(0,t)=\gamma \left(A_{10}^2\left(t\right)+2A_{10}^{*}\left(t\right)A_{30}\left(t\right)\right),\hfill \\ w_1(0,t)=-3\gamma A_{10}\left(t\right)A_{20}\left(t\right),t\in [0,L_t],\hfill \\ U(z,0)=V(z,0)=W(z,0)=U(z,L_t)=V(z,L_t)=W(z,L_t)=0,\hfill \\ u_1(z,0)=v_1(z,0)=w_1(z,0)=u_1(z,L_t)=v_1(z,L_t)=w_1(z,L_t)=0,z\in [0,L_z].\hfill \end{array}$$

(7)

The set of Equation (5) possesses some conservation laws (invariants):

$$\begin{array}{c}{I}_{1UW}=\underset{0}{\overset{L_t}{\int }}\left({|U|}^2+{|W|}^2\right)dt=const,\hfill \\ I_{1V}=\underset{0}{\overset{L_t}{\int }}{|V|}^{2}dt=const,\hfill \\ I_3=\underset{0}{\overset{L_t}{\int }}(3{\nu }_{21}Im\left(V^{*}\frac{\partial V}{\partial t}\right)+2{\nu }_{31}Im\left(W^{*}\frac{\partial W}{\partial t}\right)-6D_1{\left|\frac{\partial U}{\partial t}\right|}^2-3D_2{\left|\frac{\partial V}{\partial t}\right|}^2-2D_3{\left|\frac{\partial W}{\partial t}\right|}^2\hfill \\ -3\tilde{\alpha }\left(4Re\left(U^3{W}^{*}\right)+{|U|}^4+{4|U|}^2{|W|}^2-{8|U|}^2{|V|}^2+{2|V|}^2{|W|}^2\right))dt=const.\hfill \end{array}$$

(8)

These invariants show that, in the framework of the modified equations, the energy exchanges occur only between LFW and HFW. Meanwhile, the IFW energy remains constant. This fact explains why we choose the normalization value $A_0$ in (3) as the square root from the sum of the intensities of LFW and HFW achieved at the pulse center.

3.2. Frequency Down-Conversion in the Framework of the Long Pulse Duration Approximation

Although our primary goal was to analyze a process of the frequency down-conversion, accounting for SOD, we will briefly present an analysis of this process using the long pulse duration approximation. It allowed us to estimate maximal conversion efficiency.

Let us suppose that the SOD coefficients are equal to zero: $D_j=0,j=1,2,3$. Thus, the functions U, V, W depend only on z—coordinate. In this case, the problem (5), (7) can be rewritten as follows:

$$\begin{array}{c}\frac{dU}{dz}-i\tilde{\alpha }{(|U|}^{2}U+3U^{*2}W-{4U|V|}^2+{2U|W|}^2)=0,\hfill \\ \frac{dV}{dz}+2i\tilde{\alpha }{(4|U|}^2-{|W|}^2)V=0,\hfill \\ \frac{dW}{dz}-3i\tilde{\alpha }(U^3+{2|U|}^{2}W+{|V|}^{2}W)=0,\hfill \\ U\left(0\right)=A_{10},V\left(0\right)=A_{20},W\left(0\right)=A_{30}.\hfill \end{array}$$

(9)

The conservation laws (8) transform in the following way:

$$\begin{array}{c}{I}_{1UW}={|U|}^2+{|W|}^2=1,\hfill \\ I_{1V}={|V|}^2={|A_{20}|}^2,\hfill \\ I_3=-3\tilde{\alpha }\left(4Re\left(U^3{W}^{*}\right)+{|U|}^4+{4|U|}^2{|W|}^2-{8|U|}^2{|V|}^2+{2|V|}^2{|W|}^2\right)=const.\hfill \end{array}$$

(10)

The energy invariant $I_{UW}$ is chosen equal to unity, for definiteness. This invariant’s choice leads to more simple formulas for LFW generation/amplification efficiency. In general, this value is easy to realize by renormalization of the complex amplitudes.

The Equation (9) can be reduced to a single differential equation. For this aim, we represent the complex amplitudes in a standard way:

$$U\left(z\right)=a_1\left(z\right)expi{\phi }_1\left(z\right),V\left(z\right)=a_{20}exp\left(i{\phi }_2\left(z\right)\right),W\left(z\right)=a_3\left(z\right)exp\left(i{\phi }_3\left(z\right)\right),$$

(11)

here, the functions $a_j,{\phi }_j,j=1,2,3$ are real-valued functions. We notice that an equality of $a_{20}=|A_{20}|$ takes place because of the IFW energy preservation. Thus, the problem (9) takes the form

$$\begin{array}{c}\frac{d{a}_1}{dz}=-3\tilde{\alpha }{a}_1^2{a}_{3}sin\phi ,\hfill \\ \frac{d{a}_3}{dz}=3\tilde{\alpha }{a}_1^{3}sin\phi ,\hfill \\ \frac{d\phi }{dz}-\tilde{\alpha }\left(3\left(\frac{a_1^3}{a_3}-3a_1{a}_3\right)cos\phi +3a_1^2-6a_3^2+15a_{20}^2\right)=0,\hfill \\ \frac{d{\phi }_2}{dz}+2i\tilde{\alpha }(4a_1^2-a_3^2)=0,\hfill \\ a_1\left(0\right)=|A_{10}|,a_3\left(0\right)=|A_{30}|,\phi \left(0\right)={\phi }_0,{\phi }_2\left(0\right)=arg\left(A_{20}\right).\hfill \end{array}$$

(12)

Here, $\phi ={\phi }_3-3{\phi }_1$ is a phase difference between HFW and LFW, ${\phi }_0$ is its value in the input section of a medium. Obviously, the invariants (10) are transformed to a form:

$$\begin{array}{c}{I}_{1_{a_1{a}_3}}=a_1^2+a_3^2=1,\hfill \\ I_{1_{a_2}}=a_2^2=a_{20}^2,\hfill \\ I_3=3\tilde{\alpha }\left(-4a_1^3{a}_{3}cos\phi -a_1^4-4a_1^2{a}_3^2+8a_{20}{a}_1^2-2a_{20}^2{a}_3^2\right).\hfill \end{array}$$

To write the algebraic equation with respect to the phase difference, we modify Hamiltonian by dividing it on $3\tilde{\alpha }$:

$${\tilde{I}}_3=-4a_1^3{a}_{3}cos\phi -a_1^4-4a_1^2{a}_3^2+8a_{20}{a}_1^2-2a_{20}^2{a}_3^2={\tilde{I}}_{30}$$

(13)

Thus, we can express $cos\phi$ from the Hamiltonian (13):

$$cos\phi =\frac{2a_{20}^2(4a_1^2-a_3^2)-{\tilde{I}}_{30}-a_1^4-4a_1^2{a}_3^2}{4a_1^2{a}_3^2}$$

(14)

Substituting the expression (14) into the first equation of the set (12), we obtain the equation with respect to the LFW amplitude $a_1$:

$$\frac{d{a}_1}{dz}=\mp \tilde{\alpha }{a}_1^2{a}_3\sqrt{1-\frac{(2a_{20}^2(4a_1^2-a_3^2)-{\tilde{I}}_{30}-a_1^4-4a_1^2{a}_3^2)}{16a_1^6{a}_3^2}}.$$

Multiplying both parts of the equation on $a_1$, and using a new notation $p_1=a_1^2$ (it means the LFW intensity), we write the differential equation with respect to the intensity of the LFW $p_1$, accounting for an equality $a_3^2=1-p_1$:

$$\begin{array}{c}\frac{d{p}_1}{dz}=\mp 7.5\tilde{\alpha }\sqrt{f\left(p_1\right)},\hfill \\ f\left(p_1\right)=-p_1^4+(0.64+0.48B)p_1^3+(0.24A-0.16B^2)p_1^2-0.16AB{p}_1-0.04A^2,\hfill \\ A={\tilde{I}}_{30}+2a_{20}^2,B=2-5a_{20}^2.\hfill \end{array}$$

(15)

The maximal LFW intensity is defined by the roots of the equation $f\left(p_1\right)=0$. As neither parameter A nor parameter B depend on γ and ${\Delta }_{21}k$, the maximal LFW intensity depends only on the incident intensities of interacting waves. Obviously the nonlinear coupling coefficient and phase mismatching ${\Delta }_{21}k$ influence only on a distance on which the maximal LFW intensity achieves.

Since we want to choose the intensity of incident LFW that is as small as possible, the function $p_1\left(z\right)$ should achieve its minimum in section $z=0$. Therefore, its derivative must be equal to zero. As follows from the first Equation (12), this means either ${\phi }_0=0$ or ${\phi }_0=\pi$. Under this assumption, we solve the equation $f\left(p_1\right)=0$ for various values $|A_{10}{|}^2,{|A_{20}|}^2$ and depict the results of the computation on the plane ($|A_{10}{|}^2,{|A_{20}|}^2$) (Figure 1).

Thus, one can see that there are two regimes of the frequency conversion: low-efficient and high-efficient. In the first one, the conversion efficiency is lower than 20%; in the second one, the conversion efficiency is much higher and can be higher than 90%. We could also see in Figure 1 that if the intensity of incident IFW equals zero then the intensity of incident LFW must be greater or equal than 0.08: $|A_{10}{|}^2\ge 0.08$ to achieve the high-efficiency mode of the frequency conversion. Thus, in accordance with data from Table 1, the following incident intensities of the LFW and HFW are enough for the high-efficient amplification of the pulse with the 4 μm wavelength: 0.4976 GW/cm² and 5.7224 GW/cm². If the intensity of incident LFW is lower, then the amplification efficiency decreases significantly.

However, with the increasing incident of the IFW intensity, the incident LFW intensity that is required to achieve the high-efficiency mode of the frequency conversion decreases. Moreover, if the incident IFW intensity is equal to $|A_{20}{|}^2=0.4$, then the high-efficiency mode occurs even for a zero-value of the incident LFW intensity. The IFW and HFW incident intensities, corresponding to these dimensionless values, can be the following: 2.488 GW/cm² and 6.22 GW/cm².

It should be noted that the computer simulation results obtained by solving the original problem mostly support this analysis provided on the basis of the modified equations. In particular, two different modes of the frequency conversion also occur if we describe the laser pulse interactions in the framework of the original problem (1).

4. Computer Simulation Results

To confirm the results, discussed in the previous paragraph, the computer simulation results obtained on the basis of solving the problem (1), are presented below. The red solid lines refer to LFW; the blue solid lines refer to IFW; the green solid lines refer to HFW; the black solid lines with triangles denote the incident LFW intensity; the black dashed-dotted lines denote the IFW intensity; the black dashed lines denote the incident HFW intensity. We also placed numbers near the curves: 1—LFW, 2—IFW, 3—HFW.

The distributions of the complex amplitudes for the incident pulses are chosen as:

$$A_{j0}\left(t\right)=A_{j0}exp(-{(t-0.5L_t)}^2),j=1,2,3.$$

(16)

The intensities of LFW and HFW are satisfied to equality: $|A_{10}{|}^2+{|A_{30}|}^2=1$. We also estimate the conversion efficiency via the following formula:

$${\eta }_j=\frac{\underset{0}{\overset{L_t}{\int }}{|A_j(z,t)|}^{2}dt}{\underset{0}{\overset{L_t}{\int }}(|A_1{(0,t)|}^2+|A_2{(0,t)|}^2+|A_3(0,t){|}^2)dt},j=1,2,3.$$

4.1. Frequency Conversion to Radiation with the Wavelength 4 μm

Here, we present the computer simulation results of the energy conversion from HFW to LFW, possessing wavelength 4 μm, occurring in the crystal AgGaS₂. The SOD coefficients are chosen as follows: $D_1=-0.0002,D_2=-0.0125,D_3=-0.0217$. So, the frequency of LFW is near the zero-dispersion point and the SOD of the HFW is a large one. In our notations, the negative sign of the SOD coefficient corresponds to the normal dispersion of a medium. The coefficient of nonlinear coupling γ is chosen equal to unity, which is achieved at a value of 6.12 GW/cm² of the sum intensity of the incident pulses.

4.1.1. Incident IFW’s Intensity Is Equal to Zero

We begin our consideration from the case for which a non-zero value of the intensities of incident LFW and HFW takes place (of course, the HFW possesses much more energy, than LFW), meanwhile, the intensity of incident IFW is absent: $|A_{20}{|}^2=0$. In this case, we analyze an influence of the intensity ratios between LFW and HFW on the effectiveness of energy conversion.

First, we consider the positive phase mismatching between LFW and IFW (${\Delta }_{21}k=20$). Figure 2 presents the computer simulation results for various maximal intensities of the incident LFW: $|A_{10}{|}^2=0.05,0.07,0.08,0.1$. We emphasize that the first two values of the intensity lead to the low-effective mode of the frequency down-conversion, and the two last values—to its high-effective mode.

Indeed, at the incident intensity $|A_{10}^2|=0.05$, there is no remarkable frequency conversion between HFW and LFW (Figure 2i): ${\eta }_1$ grows from 5% only to 7%. The LFW intensity at the pulse center also grows a little bit (Figure 2e). As for the shapes of the pulses (Figure 2a), the LFW pulse shape becomes flatter than the initial one, and the HFW pulse decompresses due to the SOD influence. Moreover, a weak IFW generation occurs (as it is supposed to).

The same situation is practically observed in the two next cases. At $|A_{10}{|}^2=0.07$, the frequency conversion is slightly more effective: ${\eta }_1$ grows two times; from 7% to 15% (Figure 2j). Other peculiarities, such as the LFW intensity growth at the pulse center (Figure 2f), flattening of the LFW pulse shape, the HFW pulse decompression, and weak IFW generation (Figure 2b), are conserved. The incident intensity $|A_{10}{|}^2=0.08$ does not experience enough improvement of the frequency down-conversion (${\eta }_1$, achieving only 19% (Figure 2k)) in contrast to those achieved in the framework of the long-duration pulse approximation.

The explosive increasing frequency conversion efficiency occurs at $|A_{10}{|}^2=0.1$. In this case, the LFW intensity at the pulse center (Figure 2h) rises much faster than in all previous cases and even achieves the incident HFW intensity. Moreover, the LFW pulse (Figure 2d) is a bit more narrow than the incident HFW one.Thus, the resulting frequency conversion is very impressive: more, than 69% of the sum energy transfers to LFW (Figure 2l). It is worth noting that the HFW pulse has a local minimum near the pulse center, in this case (Figure 2d).

If we take into account the GVDs of the optical pulses, then a sign of the phase mismatching ${\Delta }_{21}k$ will influence the conversion efficiency. So, if we choose a negative (${\Delta }_{21}k=-20$), then the situation changes, essentially because an action of a medium leads to decompression of the interacting pulses due to changing of the effective nonlinear response (see above: $\tilde{\alpha }={\gamma }^2/{\Delta }_{21}k$). Because the GVD coefficient $D_1$ of the LFW is considerably small, this pulse undergoes decompression very weakly. As a consequence, the energy from the central part of the HFW converts to the energy of LFW, and the LFW intensity at the pulse center becomes larger than those occurring for ${\Delta }_{21}k=20$ (compare Figure 3e–h with Figure 2e–h). However, the pulse of HFW spreads faster, and most of it locates out of the time interval in which two other pulses are located. Consequently, no remarkable frequency conversion occurs far from the pulse centers. Thus, the HFW pulse possesses a local minimum near the pulse center in all cases (Figure 3a–d) despite the LFW pulse being smooth, with a small duration in comparison with the HFW pulse duration. The conversion efficiency is larger in the first three cases (18%, 34%, 38% in Figure 3i,j,k, correspondingly), but lower for the incident intensity of the LFW equal to $|A_{10}{|}^2=0.1$ than the one occurring for the positive phase mismatching: ${\Delta }_{21}k=20$ (only 43%).

4.1.2. Incident LFW’s Intensity Is Equal to Zero

Below, we briefly discuss peculiarities of the frequency down-conversion if the incident LFW intensity is equal to zero ($|A_{10}{|}^2=0$), and the intensity of the incident IFW is non-zero ($|A_{20}{|}^2=0.4$, for instance). In this case, at $\gamma =1$, a much longer distance ($z=80$) of the pulses’ interaction is required for the LFW generation. Obviously, the required distance can be decreased by the incident intensity increasing. For example, at $\gamma =2$, the distance decreases five times, but the frequency down-conversion occurs in the same way as at $\gamma =1$: there are no improvements in the pulse shapes.

The main feature of the interactions of the pulses involve developing their instability, which destroys the pulse shapes. Therefore, this scheme involving the pulse interactions at chosen parameters cannot be effectively used.

As above, a sign of the phase mismatching ${\Delta }_{21}k$ remarkably influences the frequency down-conversion process, but the pulse shapes do not remain smooth. If ${\Delta }_{21}k$ is positive, then the IFW energy converts partially to the LFW’s one. The conversion efficiency of the frequency down-conversion is about 24%. If the phase mismatching between LFW and IFW is negative, then the LFW generation is weaker than in the previous case (${\eta }_1=0.12$), and the IFW amplification occurs.

It should be noted that, in contrast to the frequency conversion in the crystal AgGaS₂, for the tellurium crystal, we observe a completely different situation, as one can see below.

4.2. Frequency Conversion to Radiation with the Wavelength 10 μm

If the LFW’s wavelength equals 10 μm, then the dimensionless SOD coefficients are equal to $D_1=0.1633,D_2=0.0755,D_3=-0.0414$ for the crystal AgGaS₂, respectively. Thus, the HFW undergoes a normal dispersion, and the LFW and IFW undergo anomalous ones. In this case, LFW amplification is not monotonic as in the previous case.

A significant increase of the conversion efficiency can be achieved by increasing the nonlinear coupling coefficient γ up to 4 to decrease the crystal length. In this case, the sum incident pulses intensity has to equal 330 GW/cm², keeping in mind the changing of the wavelength, increasing the coefficient γ, and changing the quadratic susceptibility due to changing the wavelength. It should be noted that this value is relatively high and perhaps requires an account for the influence of the third-order susceptibility on the three pulse interactions. Our computation shows that the dimensionless third-order nonlinear coefficient is equal to 0.02 in the case under consideration. Therefore, analyzing laser pulse interactions in short distances, the third-order nonlinear effects can be neglected.

The computer simulation results are depicted in Figure 4 for the phase mismatching between IFW and LFW equaling ${\Delta }_{21}k=22$.

As one can see, there is a very effective generation of the IFW, although this wave is not phase-matched with two other waves in this case (Figure 4a). The LFW amplification efficiency achieves 41% and the intensive energy conversion to this wave occurs between sections $z=2$ and $z=3$, including the explosive energy conversion of the interacting waves. Then the energy exchange between the interacting waves becomes very small. Unfortunately, the pulse shapes have many local maxima and minima, which make the use of this mode of wave interactions for the frequency down-conversion impossible, in practice. It should be stressed that at a smaller incident intensity of the LFW ($|A_{10}{|}^2$), the process of the frequency conversion takes place in the same manner, but with lower efficiency.

There is a similar conclusion with the LFW. The pulse shapes are also not smooth, and the HFW energy transfers to both LFW and IFW (Figure 4b). As a result, the frequency down-conversion efficiency achieves 21%.

The quality of the pulse shape and the frequency conversion efficiency can be sufficiently improved by increasing the incident pulse duration, for instance, until ${\tau }_P=1$ ps. This leads to decreases in the dimensionless GVD coefficients, for 100 times, and allows us to avoid developing the modulation instability of the pulses (Figure 4c,d). We see in this figure that even at a smaller value of the nonlinear coupling coefficient ($\gamma =1$) corresponding to the incident intensity 20.66 GW/cm², the conversion efficiency achieves a value of about 76% (Figure 4d). However, it requires increasing the length of the crystal: about 4 cm.

4.3. Frequency Conversion to Radiation with the Wavelength to 24 μm

Finally, we consider the frequency down-conversion process in a tellurium crystal at the incident pulse duration, 100 fs, which results in radiation generation with a frequency of 12.5 THz, corresponding to a wavelength of 24 μm. The phase mismatching between IFW and LFW is small: ${\Delta }_{21}k=5.2$. Therefore, the multi-scale method can give non-adequate results. However, some features of those analyses remain valid. The dimensionless SOD coefficients are also large, especially at the wavelength 24 μm ($D_1=0.218$, $D_2=-0.079$, $D_3=-0.154$). Consequently, we chose the coefficient of nonlinear coupling equal $\gamma =2$. Due to the large value of the quadratic susceptibility ${\chi }^{\left(2\right)}$ of the tellurium crystal, the corresponding sum intensity of the incident pulse can be small enough: 110 MW/cm². The computer simulation results are shown in Figure 5.

As one can see, the high- and low-effective modes of the frequency conversion can be observed in this figure. At the incident intensity $|A_{10}{|}^2=0.07$ of the LFW, its energy changes from 7% to 34% (Figure 5g) and the pulse duration is about 200 fs (Figure 5a), which approximately corresponds to three periods of wave phase changes. Meanwhile, if the incident intensity slightly increases, up to $|A_{10}{|}^2=0.08$, then the conversion efficiency ${\eta }_1$ achieves more than 82% (Figure 5h) and the pulse duration becomes equal, at about 500 fs (Figure 5b), which approximately corresponds to eight periods of wave phase changes. It is very important for practice that the LFW pulse shape is rather smooth (Figure 5a,b) in contrast to the two other waves.

If the incident LFW intensity is equal to zero, then the conversion efficiency achieves about 21% (Figure 5i) and the pulse duration is about 250 fs (Figure 5c), which corresponds to 4.5 periods of wave phase changes, approximately. However, the LFW pulse shape contains some local maxima and local minima. Nevertheless, its shape is smooth enough (Figure 5c).

In Figure 5d–f, we depict the spectrum of the LFW. In the first two cases (Figure 5d,e), the LFW spectrum is smooth and broadened compared to the incident pulse. Regarding the LFW generation from its incident zero-value intensity (Figure 5f), the LFW spectrum has three local maxima. Thus, one could analyze the three sub-pulses, as could be seen in Figure 5c; they overlap each other in the time-domain.

The chirps of the incident pulses:

$$A_{j0}\left(t\right)=A_{j0}exp(-{(t-0.5L_t)}^2+i{c}_j{(t-0.5L_t)}^2),j=1,2,3$$

can partially improve the frequency down-conversion efficiency. Above $c_j$ equals to −1, 1, or 0. We made a series of the computer simulations for the parameters: $|A_{10}{|}^2=0.07,$ $|A_{20}{|}^2=0,$ $\gamma =2,{\Delta }_{21}k=5.2,D_1=0.218,D_2=-0.079,D_3=-0.154$, at which the frequency down-conversion is relatively small; a quality of the pulse shape is bad for non-chirped pulses (see Figure 5a,d,g). For comparison, the computer simulation results are presented in Figure 6.

It should be noted that both the up-chirping ($c_3=1$, Figure 6a,d,g) and the down-chirping ($c_3=-1$, Figure 6b,e,h) of the HFW pulse lead to sufficient improvements of the frequency down-conversion efficiency—about 70% is achieved in both cases (compared with the 34% conversion efficiency in Figure 5g). However, there are some differences between these two cases of the LFW generation. The mentioned conversion efficiency is achieved for the down-chirped HFW pulse in a two-times smaller distance ($z=5$) than the corresponding value occurring for the up-chirped pulse of the HFW ($z=10$). If the pulse chirp is $c_3=1$, then the pulse shapes are smoother (Figure 6a) and do not possess the local minima, which can be observed in Figure 6b for IFW and HFW. However, the LFW pulse spectrum is broadened if the incident pulse possesses down-chirp ($c_3=-1$): the remarkable response of a medium can be observed in the pulse spectrum up to dimensionless frequencies $\omega =\pm 6$ in Figure 6e, meanwhile, the LFW pulse spectrum almost vanishes at the frequency $\omega =\pm 3$ in Figure 6d.

The effective LFW amplification also occurs if both the LFW and HFW possess down-chirps $c_1=-1,c_3=-1$ in the input section $z=0$ (Figure 6c,f,i). In general, the frequency conversion process in this case is similar to those occurring for the pulse chirps $c_1=0$, $c_3=-1$ (Figure 6b,g,h). Only a slightly longer distance $z=6$ is required to achieve the high efficiency of the frequency conversion (Figure 6h) and a more pronounced spectral response occurs at a range of the dimensionless frequencies $\omega =\pm (2.5-6.5)$ (Figure 6f).

5. Discussion and Conclusions

We propose using the cascading process for frequency down-conversion to the mid-infrared (or even THz) range, due to wave generation with difference frequency at multiple frequencies of the interacting pulses. We showed that this method is applicable for frequency down-conversion corresponding to a wavelength of at least 24 μm, but this is not a strict ’upper bound’.

In the framework of a multi-scale method, we derived a set of modified equations and solved these equations without using the energy non-depletion approximation of the pump wave. This solution was supported by numerical experiments.

Influence of the GVD—of the pulses on the frequency down-conversion efficiency—was examined. The computer simulation results showed that non-zero incident LFW’s energy could be amplified from an initial value of 8% to 75% and the LFW generation with 25% conversion efficiency is possible at the zero-value its incident intensity. It is important (for practice) that the pulse with a larger wavelength possesses a smooth shape and that its spectrum is also smooth.

Chirping of the incident HFW pulse could increase the conversion efficiency if the pulse chirp is chosen in an appropriate way. The significant increasing is observed for both up- and down-chirping of the pulse.

Concerning the possible experimental setup, based on data from Table 1 and computer simulation results—for the amplification of the optical pulse with the wavelength 4 μm, we suggest the following configuration: two pulses, approximately with 100 fs durations, and the intensities of 0.612 GW/cm² (10% of the sum intensity) and 5.508 GW/cm² (90% of sum intensity), with wavelengths ${\lambda }_1=4$ μm (75 THz) and ${\lambda }_3\approx 1.333$ μm (225 THz), respectively, fall on the AgGaS₂ crystal with the length 4 cm, cut at an angle 49.46°.

For amplification of the optical pulse with 10 μm wavelength, the crystal cut angle should be changed to 79.51°. The duration of the pulses should be increased until 1 ps and the intensities between them should be distributed in the following way: 2.066 GW/cm² for the pulse with the wavelength ${\lambda }_1=10$ μm (30 THz) and 18.54 GW/cm² for the pulse with the wavelength ${\lambda }_3\approx 3.333$ μm (90 THz).

The experimental setup for a pulse generation with the wavelength 24 μm can be implemented in the following way: the Te crystal, 2.5 mm in length, should be cut at an angle, 15.78°. Two pulses with 100 fs duration and with intensities of 0.44 GW/cm² at the wavelength ${\lambda }_3=8$ μm (73.5 THz) and 0.176 GW/cm² at the wavelength ${\lambda }_2=12$ μm (49 THz) should ‘fall’ on the crystal.

For the frequency down-conversion of the radiation with a wavelength λ = 1.3 (or 1.1) μm to the wavelength λ = 24 (or 30) μm, we propose, for example, two schemes (Figure 7) that allows us to reach the frequency 12.5 THz (Figure 7a) and 10 THz (Figure 7b), respectively. For this aim, it is necessary to use three crystals. In the first crystal (AgGaS₂), a radiation with the tripled wavelength 4 μm is generated. Then, the second similar crystal is used for the generation of a radiation with the wavelength 8 μm or 10 μm. The generation of the radiation with wavelength 24 μm or 30 μm occurs in the third crystal (Te or Cs₂HgI₂Cl₂).

In above consideration, we did not take into account the absorption of laser radiation because our aim was a study of a maximal efficiency of the down-frequency based on the cascaded processes. If this efficiency was to be small, then, evidently, it would not make sense to consider other physical factors that decrease its effectiveness. One of these factor is the crystal’s absorption of the laser radiation in the far IR and THz range of frequencies. Two crystals, used in our computer simulation, possess the following absorption coefficients for the radiation with wavelengths 4 mm and 10 mm: about 1.2 cm⁻¹ for the crystal AgGaS₂ [44]; and for the radiation with wavelength 24 mm: about 1.7 cm⁻¹ for the crystal Te [36]. In dependence of a ratio between the intensities of the incident pulses the required crystals’ lengths can change in the interval (2 mm, 7 mm) or or even longer if the nonlinear coupling coefficient γ is equal to unity. To decrease the absorption of the laser energy, one can increase the intensity of the incident pulses that it is possible because we used the low-intensive pulses. In this case, we can decrease the crystal length in two or even more times. Moreover, there is other possibility to decrease the laser energy losses caused by the absorption by the crystals.At present time, many new nonlinear crystals were developed and they are transparent up to the wavelength 31 μm (Cs₂Hg₃I₈, [45]), 41 μm (Cs₂HgI₂Cl₂, [46]), respectively, or even 50 μm (6 THz, Cs₂Hg₂Br₂I₄·H₂O, [47]) (full review of this research can be seen in [48]).

It should be mentioned that there are various IR laser, such as CO₂ lasers with the wavelength 10.6 μm and the duration 200 ns [49], the fiber lasers with the wavelength 3.9 μm and with the pulse duration 160 fs with maximal power 200 kW [50,51], the quantum cascade laser that can generate a pulse with the wavelength ${\lambda }_1=8$ μm and with the pulse duration up to 630 fs possessing maximal power $maxP\left(t\right)$ about of 4.5 W [52] and some others. Our scheme of the frequency down-conversion allows us to obtain the pulse with shorter duration and various wavelength and possessing broadband spectrum and with much high power density. Therefore, this scheme supplements the existence sources of the IR radiation and can be used for a generation of the THz broadband pulse.

Additional remark about the application of the converted frequency to the THz of the frequencies. As a rule, the THz radiation refers to the range of frequencies belonging to interval 0.1–10 THz. Figure 7 illustrates how one can reach this frequency range by using proposed approach. One can also use the quantum cascade laser and sources of the IR pulsed radiation and the chosen crystal for the frequency down-conversion. We emphasize that the many dangerous substances have the absorption frequencies in the range of the frequencies 10–20 THz (see, for example, [53], Table 1 in [54], Table 9.1 in [55], Figure 1 in [56]. Evidently, that these frequencies can be used for the problem of the detection and identification of such substances that is very important for practice. Thus, the proposed scheme of the frequency down-conversion can be covered this frequency range.