# The Quantum Analysis of Nonlinear Optical Parametric Processes with Thermal Reservoirs

Authors: Tamirat Abebe; Nebiyu Gemechu; Chimdessa Gashu; Kebede Shogile; Solomon Hailemariam; Shimelis Adisu
Journal: International Journal of Optics
 (2020)

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## Abstract

In this paper, employing the stochastic differential equations associated with the normal ordering, the quantum properties of a nondegenerate three-level cascade laser with a parametric amplifier and coupled to a two-mode thermal reservoir are thoroughly analyzed. Particularly, the enhancement of squeezing and the amplification of photon entanglement of the two-mode cavity light are investigated. It is found that the two cavity modes are strongly entangled and the degree of entanglement is directly related to the two-mode squeezing. Despite the fact that the entanglement and squeezing decrease with the increment of the mean photon number of the thermal reservoir, strong amount of these nonclassical properties can be generated for a considerable amount of thermal noise with the help of the nonlinear crystal introduced into the laser cavity. Moreover, the squeezing and entanglement of the cavity radiation enhance with the rate of atomic injection.


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## Body

## 1. Introduction

Three-level cascade lasers have received considerable interest in connection with its potential as a source of light with interesting nonclassical features [1–6]. The quantum properties of the light is attributed to atomic coherence that can be induced either by preparing the atoms initially in a coherent superposition of the top and bottom levels [7] or coupling these levels by an external radiation [8] or using these mechanisms together [9].Moreover, some authors have studied quantum properties of light generated by the three-level laser whose cavity contains a parametric amplifier [10–13]. A parametric amplifier involves three different modes of the radiation field, the signal, the idler, and the pump which are coupled by a nonlinear medium. In these devices, a pump photon interacts with a nonlinear crystal inside a cavity and is down converted into two highly correlated photons of different frequencies [12]. These works indicated the cavity radiation is found to be in squeezed and entangled states under certain conditions. In addition, the mean and variance of the photon number for a degenerate [11–13] and nondegenerate [14–19] three-level cascade laser whose cavity contains a parametric amplifier have been determined for different cases.Furthermore, Tesfa [20] studied a two-photon correlated emission laser (CEL) in which the atomic coherence is initially prepared and the cavity is coupled to a two-mode thermal reservoir via a single-port mirror. He analyzed the effects of decoherence on entanglement in the two modes and evaluated the inseparability criterion for a continuous Gaussian state proposed earlier by Duan et al. [21]. He found that the generated light exhibits a two-mode squeezing and entanglement when initially there are more atoms at the lower level, even when the cavity is coupled to a thermal reservoir. Moreover, he also found that though the thermal noise entering the cavity degrades the squeezing and entanglement, it significantly increases the mean number of photon pairs of the superimposed radiation.Moreover, Tesfa [22] studied the effect of the thermal light initially seeded in the cavity on the statistical and quantum features of the cavity radiation, but in the absence of the parametric amplifier. Thus, it has been shown that the degree of two-mode squeezing is almost independent of which mode is initially seeded, but the degree of entanglement decreases considerably when a light with the same strength is seeded in mode b. Moreover, the thermal light significantly damages two-mode squeezing and entanglement in the earlier stages of the lasing process. Thus, it is worthwhile to investigate the effect of thermal noise on these very sensitive nonclassical properties. On the other hand, the squeezing, entanglement, and statistical properties of the cavity radiation can be enhanced with the introduction of the parametric amplifier into the laser cavity. With this motivation, we are devoted to investigate the nonclassical properties of the light generated by a nondegenerate three-level laser whose cavity contains a nondegenerate parametric amplifier and coupled thermal reservoir.In this study, the squeezing, entanglement, and statistical properties of the light produced by a nondegenerate three-level laser with a nondegenerate parametric amplifier and coupled to thermal reservoir are studied. We consider a nondegenerate three-level laser in which the pump mode emerging from the parametric amplifier does not couple the top and bottom levels of the injected atoms [17]. We carry out our analysis applying the pertinent master equation describing the dynamics of the optical device. The solutions for c-number cavity mode variables and correlation property of noise forces associated with normal ordering are determined. Using the resulting solutions and steady-state consideration, we obtained quadrature squeezing, the photon entanglement, the mean number of photon pairs, Mandel’s Q-factor, and the second-order correlation functions of the two-cavity mode variables.The paper is organized as follows. In the second section, the Hamiltonian and the model are presented, the master equation describing the dynamics of the optical device is derived, and the solutions of the cavity-mode variables are determined. The squeezing and entanglement of the two-mode cavity radiation are analyzed in the third and fourth sections. In the fifth section, the statistical properties of the cavity radiation such as mean photon number, Mandel’sQ-factor, and photon number correlation are studied.


## 2. Hamiltonian and Master Equation

We represent the top, intermediate, and bottom levels of a three-level atom in a cascade configuration by3, 2, and 1, respectively, as shown in Figure 1. In addition, we assume the two modes a1 and a2 to be at resonance with the two transitions 3⟶2 and 2⟶1 dipole allowed, respectively, and direct transition between level 3 and level 1 to be dipole forbidden. The interaction of a nondegenerate three-level atom with the cavity modes can be described by the Hamiltonian in the interaction picture with the rotating and electric dipole approximation as(1)H^I=ig32a^1−a^1†23+21a^2−a^2†12,where g is a coupling constant, which is taken to be the same for both transitions, and a^1 and a^2 are the annihilation operators for the two cavity modes.Figure 1
Schematic representation of a two-mode three-level cascade laser coupled with a two-mode thermal reservoir.In this paper, we take the initial state of a three-level atom to beψA0=C303+C101, and hence, the initial density operator for a single atom has the form(2)ρ^A0=ρ33033+ρ31031+ρ13013+ρ11011,where ρ330=C32 and ρ110=C12 are, respectively, the probabilities for the atom to be initially in the upper and lower levels, and ρ310=C3C1∗ and ρ130=C1C3∗. Actually, this assumption corresponds to a situation in which the three-level atom is initially prepared in a coherent superposition of the top and bottom levels. Experimental demonstration of coherent superpositions of the top and bottom levels of the atom was studied by Calderin et al. [23].In addition, we seek to consider when such atoms are injected into a cavity at constant ratera and removed after sometime τ, which is long enough for the atoms to decay spontaneously to levels other than the middle or the lower level. The spontaneous decay rate γ is taken to be the same for the two upper levels. In the good cavity limit, γ≫κ, where κ is the cavity damping constant, the cavity mode variables change slowly compared with the atomic variables. Hence, the atomic variables will reach steady state in relatively short time. The time derivative of such variables can then be set to zero, while keeping the remaining terms at time t. This procedure is referred to as the adiabatic approximation scheme. Since the coupling constant is taken to be small, we restrict ourselves to a linear analysis that amounts to dropping the higher order terms in g. Employing the linear and adiabatic approximation schemes in the good cavity limit that the equation of evolution of the density operator for the cavity modes has, in the absence of damping through the coupled mirror, the form [16](3)ρ^˙1t=Aρ33022a^1†ρ^a^1−a^1a^1†ρ^−ρ^a^1a^1†+Aρ11022a^2ρ^a^2†−a^2†a^2ρ^−ρ^a^2†a^2−Aρ31022a^2ρ^a^1−ρ^a^1a^2−a^1a^2ρ^−Aρ13022a^1†ρ^a^2†−ρ^a^1†a^2†−a^1†a^2†ρ^,where A=2g2ra/γ2 is the linear gain coefficient and for convenience we have set ρ310=ρ310∗.In order to study the dynamics of the cavity radiation of the combined system, it is necessary to obtain the corresponding equations of evolution. To begin with, the contribution of the initial thermal light in the cavity and the two-mode vacuum reservoir to the master equation are sought. To this end, one can start with the well-established fact that the time evolution of the reduced density operator for the cavity radiation coupled to a reservoir has, in the Born approximation [16], the form(4)ρ^˙2t=−iH^St,ρ^t−iH^SRtR,ρ^0−∫0tρ^SRtR,H^St′,ρ^t′dt′−∫0tTrRH^SRt′,H^SRt′,ρ^t′R^dt′,where S and R refer to the system and reservoir variables and ρ^0 represents the radiation initially in the cavity. Here, we consider the reservoirs to be composed of large number of submodes. Thus, the interaction of a two-mode cavity radiation with a two-mode thermal reservoir can be described in the interaction picture by a Hamiltonian of the form(5)H^SR=i∑jλja^1†a^1jeiω0−ωjt−a^1a^1j†e−iω0−ωjt+a^2†a^2jeiω0−ωjt−a^2a^2j†e−iω0−ωjt,where ω0=ω1+ω2/2, with ω1 and ω2 representing the frequencies of the cavity radiations, a^1j,a^2j are the annihilation operators of the two-mode thermal reservoir, ωj is the frequency, and λj is the coupling constant for the jth mode of the reservoir. With the aid of equation (5), one can write(6)H^SRR=i∑jλja^1†a^1jReiω0−ωjt−a^1a^1j†Re−iω0−ωjt+a^2†a^2jReiω0−ωjt−a^2a^2j†Re−iω0−ωjt.Using the density operator of the thermal reservoir,(7)R^=∑n=0∞n¯thn1+n¯thn+1nn,one can easily obtain(8)a^1jR=a^2jR=a^1j2R=a^2j2R=0,(9)a^1j†a^2jR=a^2j†a^1jR=0,(10)a^1ja^2jR=a^2j†a^1j†R=0,(11)a^1j†a^a1jR=a^2j†a^a2jR=n¯th.In addition, with the help of equation (11) along with the commutation relation a^1j,a^1j†=a^2j,a^2j†=1, one obtains a^1ja^1j†=a^2ja^2j†=n¯th+1, where n¯th1=n¯th2=n¯th is the mean photon number of the thermal light. In view of these results, equation (6) reduces to(12)H^SRR=0.Therefore, the second commutation relation described in equation (4) is found to be zero. This confirms that the thermal light in the cavity does not directly contribute to the master equation. As a result, solving the remaining terms by following the standard approach yields(13)ρ^˙2t=−iH^S,ρ^t+κ2n¯th2a^1†ρ^a^1−a^1a^1†ρ^−ρ^a^1a^1†+κ2n¯th2a^2†ρ^a^2−a^2a^2†ρ^−ρ^a^2a^2†+κ2n¯th+12a^1ρ^a^1†−a^1†a^1ρ^−ρ^a^1†a^1+κ2n¯th+12a^2ρ^a^2†−a^2†a^2ρ^−ρ^a^2†a^2.In addition, in the nondegenerate three-level laser a pump mode photon of frequencyω=ω1+ω2 directly interacts with the nondegenerate parametric amplifier (NDPA) to produce the signal-idler photon pairs having the same frequencies as the two cavity modes [16, 17]. The interaction of the driving light modes, treated classically, with cavity modes, and the interaction of three-level atoms with a nondegenerate parametric amplifier can be described in the interaction picture by the quantum Hamiltonian.(14)H^S=iε1a^1†−a^1+a^2†−a^2+iε2a^1†a^2†−a^1a^2,where ε1 is proportional to the amplitude of the driving light modes and ε is considered to be real and constant and is proportional to the amplitude of the pump mode that drives the NLC (nonlinear crystal). Taking into account equations (3) and (13) along with (14), the master equation of the system turns out to be(15)ρ^˙t=ε1ρ^a^1−a^1ρ^+a^1†ρ^−ρ^a^1†+ρ^a^2−a^2ρ^+a^2†ρ^−ρ^a^2†+ε2ρ^a^1a^2−a^1a^2ρ^+a^1†a^2†ρ^−ρ^a^1†a^2†+κ2n¯th+12a^1ρ^a^1†−a^1†a^1ρ^−ρ^a^1†a^1+12Aρ330+κn¯th2a^1†ρ^a^1−a^1a^1†ρ^−ρ^a^1a^1†+12Aρ110+κn¯th+12a^2ρ^a^2†−a^2†a^2ρ^−ρ^a^2†a^2+12κn¯th2a^2†ρ^a^2−a^2a^2†ρ^−ρ^a^2a^2†+Aρ31022a^2ρ^a^1−ρ^a^1a^2−a^1a^2ρ^+Aρ13022a^1†ρ^a^2†−ρ^a^1†a^2†−a^1†a^2†ρ^.Employing this master equation, the evolution of the two-mode cavity radiation in terms ofc-number variables associated with the normal ordering α1t and α2t can be expressed in the form(16)α˙1t=−γaα1t+ν−α2∗t+ε1+f1t,α˙2∗t=−γcα2∗t+ν+α1t+ε1+f2∗t,where γa=1/2κ−Aρ110, γc=1/2κ+Aρ330, ν±=ε±1/2Aρ130, and f1t and f2∗t are the pertinent noise forces, the properties of which remain to be determined.Following the straightforward procedure outlined in [22, 24], it is possible to obtain(17)α1t=Γ+tα10+χ+tα2∗0+G1t+ζ+,(18)α2t=Γ−tα20+χ−tα1∗0+G2t+ζ−,in which(19)G1t=∫0tΓ+t−t′f1t′+χ+t−t′f2∗t′dt′,G2t=∫0tΓ−t−t′f2∗t′+χ−t−t′f1t′dt′,Γ±t=A±2λe−1/2λ∓t−A∓2λe−1/2λ±t,χ±t=2ν∓2λe−1/2λ−t−2ν∓2λe−1/2λ+t,ζ±=ε1λA+±2ν∓λ∓1−e−1/2λ∓τ−A−±2ν∓λ±1−e−1/2λ±τ,λ±=122κ+Aη±λ,A±=A±A2η2+16ε2,where the noise forces satisfy the following correlations:(20)f1t=f2t=0,f1t′f1t=f2t′f2t=0,f1∗tf2t′=f2∗t′f1t=0,f1∗tf1t′=Aρ110+κn¯thδt−t′,f2∗t′f2t=κn¯thδt−t′,f1t′f2t=122ε+Aρ130δt−t′.It proves to be useful to introduce a new parameter which relates the probabilities of the atom to be in the upper and lower levels. We define the parameterη such that ρ110=1−η/2 with −1<η<1. For three-level atoms initially in a coherent superposition of the top and bottom levels, one obtains ρ330=1+η/2, and in view of the relation ρ1302=ρ110ρ330, one easily finds ρ130=1/21−η2.


## 3. Quadrature Variance

Here, we seek to analyze the quadrature squeezing properties of the two-mode light in the cavity. The squeezing properties of the two-mode light in the cavity can be described by two quadrature operators defined as(21)c^+=c^†+c^,(22)c^−=ic^†−c^,where c^=1/2a^1+a^2 is the annihilation operator for the two-mode cavity radiation. These quadrature operators satisfy the commutation relation c^+,c^−=2i. On the basis of these definitions, a two-mode light is said to be in a two-mode squeezed state if either Δc+2<1 or Δc−2<1 [19, 24]. The variances of the quadrature operators can be expressed as(23)Δc±2=c^±2−c^±2.It is possible to express the variance of the quadrature operators (21) and (22) in terms of the c-number variables associated with the normal ordering taking the cavity modes to be initially in a two-mode vacuum state, as(24)Δc±2=1+α1∗tα1t+α2∗tα2t+2α1tα2t∓12α1∗t+α2∗t±α1t+α2t±α12t+α22t+2α1tα2t.In view of equations (17) and (18), the steady-state quadrature variances are found to be(25)Δc±2=1+κA1−η4κ+3Aη+A+16ε2κ+Aη4κκ+Aη−4ε22κ+Aη+κ4ε+A1−η24κ22κ+2Aη+A22κn¯th4κκ+Aη−4ε22κ+Aη±κ4ε+A1−η22κ+Aη+A4κκ+Aη−4ε22κ+Aη+4ε2κ+Aη+A21−η22κn¯th4κκ+Aη−4ε22κ+Aη.We clearly see from equation (25) that the quadrature variances are independent of the parameter ε1 which represents the cavity driving coherent light. This shows that the cavity driving coherent light does not have any effect on the degree of squeezing of the two-mode light. This is due to the fact that the external driving coherent light does not introduce additional coherence to the system which is believed to be the source of squeezing in three-level cascade lasers [25].As it can readily be seen from Figure2, the two-mode cavity radiation produced by a nondegenerate three-level laser with a nondegenerate parametric amplifier and coupled to thermal reservoir exhibits squeezing for some values of the injected atomic coherence. One can observe that the degree of squeezing is significantly degraded by the thermal noise. For this case, the maximum quadrature squeezing is found to be nearly 70% when the cavity is coupled to a thermal reservoir with n¯th=0 for A=100, κ=0.8, and ε=0.399 and occurs at η=0.1. Moreover, from the same figure, we observe that when the n¯th increases the degree of squeezing decreases. This is because of the effect of the thermal fluctuations arising from the heating due to vibration of the atoms on the walls of the cavity.Figure 2
Plots of the quadrature variance (equation (25)) versus η for A=100, κ=0.8, ε=0.399 and for different values of n¯th.In Figure3, we plot the variances of the minus quadrature Δc−2 versus η, the parameter for A=100, κ=0.8, n¯th=0.15, and with different values of ε. The figure clearly shows that the effect of the parametric oscillator ε is to increase the degree of squeezing for small values of η as previously determined [17].Figure 3
Plots of the minus quadrature variance (equation (25)) versus η for A=100, κ=0.8, n¯th=0.15 and for different values of ε.We clearly see from Figure4 that the degree of squeezing increases with the linear gain coefficient and a substantial degree of squeezing is found for smaller values of η. This indicates that the more the atoms are injected into the cavity at a time the more the degree of the squeezing of the cavity radiation would be. The maximum squeezing occurs when the atoms are prepared with initial coherence very close to the maximum possible value in this case. In particular, a maximum of 72% squeezing occurs at η=0.1 for A=1000, κ=0.8, ε=0.399, and n¯th=0.15.Figure 4
Plots of the minus quadrature variance (equation (25)) versus η for κ=0.8, ε=0.399, n¯th=0.15 and for different values of the linear gain coefficient.We also plotted, in Figure5, the variance of the minus squeezed quadrature versus the parameters ε and η for A=100, κ=0.8, and n¯th=0.15. It is possible to see from this plot that the two-mode squeezing increases with the amplitude of the parametric oscillator ε and for small values of η. Moreover, the value of η at which the maximum squeezing occurs decreases to zero as ε increases. Furthermore, Figure 5 clearly shows that the degree of squeezing increases due to the presence of the parametric oscillator.Figure 5
A plot of the minus quadrature variance (equation (25)) versus ε and η for A=100, κ=0.8, and n¯th=0.15.


## 4. Detection of Entanglement

For continuous variables photon entanglement, several sufficient inseparability criteria for a composite state have been proposed [21, 26–36]. The most relevant method is the logarithmic negativity which depicts the presence of entanglement for two-mode continuous variables based on the negativity of the partial transposition [22, 37, 38]. The negative partial transpose must be parallel with respect to entanglement monotone in order to obtain the degree of entanglement. The logarithmic negativity is combined with negative partial transpose in another case where VS represents the smallest eigenvalue of the simplistic matrix [22]:(26)VS=σ−σ2−4detΓ2,where the invariant and covariance matrices are, respectively, denoted as(27)σ=detΣ1+detΣ2−2detΣ12,(28)Γ=Σ1Σ12Σ12TΣ2,in which Σ1 and Σ2 are the covariance matrices describing each mode separately while Σ12 are the intermodal correlations. The elements of the matrix in equation (28) are given by(29)Γij=12X^iX^j+X^jX^i−X^iX^j,in which i,j=1,2,3,4. The quadrature operators are defined as X^1=a^1+a^1†, X^2=ia^1†−a^1, X^3=a^2+a^2†, and X^4=ia^2†−a^2. With this introduction, the extended covariance matrix, which can be expressed in terms of c-number variables associated with the normal ordering and nothing that α1α2=α1∗α2∗, goes over into(30)Γ=Λ0χ00Λ0−χχ0Δ00−χ0Δ,where Λ=2α1∗α1+1, χ=2α1α2, Δ=2α2∗α2+1 are c-number variables associated with the normal ordering. The logarithmic negativity for a two-mode state is defined as(31)EN=max0,−log2VS.The entanglement is achieved whenEN is positive within the region of the lowest eigenvalue of covariance matrix VS<1.Next on account of equation (29) along with the definitions of (31), one can readily show that(32)detΣ1=2α1∗α1+12,detΣ2=2α2∗α2+12,detΣ12=−4α1α22.It is also possible to establish that(33)detΓ=detΣ1detΣ2−detΣ12TdetΣ122.As it can be noted from Figure6, the degree of entanglement increases for smaller values of the initial preparation of atoms but decreases for larger values. It can also be seen that larger values of the linear gain coefficient produces a robust entangled light. The maximum achievable degree of entangled light in this case is 96%, and it occurs for A=1000 and η=0.02. This criterion also predicts the absence of entanglement for η=1 no matter how we manipulate the rate of atomic injection in the absence of a parametric amplifier.Figure 6
Plots of the smallest eigenvalueVS versus η for n¯th=0.15, κ=0.8, ε=0.399 and for different values of the linear gain coefficient.It is not difficult to see from Figure7 that the parametric amplifier produces a considerable degree of entangled light for very small value of the linear gain coefficient regardless of how atoms are initially prepared. The maximum achievable degree of entangled light in this case is 84.5%, and it occurs for n¯th=0, A=100, and η=0.08. Moreover, it can be seen in this figure that when the values of the mean photon number of the thermal reservoir increases, the degree of entanglement decreases.Figure 7
Plots of the smallest eigenvalueVS versus η for A=100, κ=0.8, ε=0.399 and for different values of n¯th.On the other hand, Figure8 shows that the effect of the parametric amplifier for a large value of the linear gain coefficient does not produce considerable changes to the degree of entanglement. Hence, the maximum achievable degree of entangled light in this case is 82%, and it occurs for A=100 and η=0.13. The behaviors of a nondegenerate three-level laser with a nondegenerate parametric amplifier and non-degenerate three-level laser without the parametric amplifier appear to be the same for a very large value of the linear gain coefficient (rate of atomic injection) with exception of the existence of the entanglement at the minimum atomic coherence which represents absence of photons in the cavity.Figure 8
A plot of the smallest eigenvalueVS of the two-mode cavity radiation versus A and η for κ=0.8, ε=0.399, and n¯th=0.15.Furthermore, it is clearly shown in Figure9 that for large values of the linear gain coefficient A and the parametric amplifier ε, the enhancement of the maximum possible degree of entanglement is occurred. However, for smaller values of the linear gain coefficient and the pumping mode, a robust entangled light is produced.Figure 9
A plot of the smallest eigenvalueVS of the two-mode cavity radiation versus A and ε for κ=0.8, n¯th=0.15, and η=0.1.


## 5. Photon Statistics

In this section, we seek to study the statistical properties of the cavity radiation of a three-level cascade laser, such as the mean photon number, Mandel’sQ-factor, and the normalized second-order correlation function for the system under consideration.


### 5.1. Mean Photon Number

In order to know about the brightness of the generated light, it is necessary to study the mean number of photon pairs describing the two-mode cavity radiation that can be defined as(34)N¯=c^†tc^t.It then follows that(35)N¯=12α1∗tα1t+α2∗tα2t.Sinceα1∗tα1t and α2∗tα2t represent the mean photon numbers in mode a1 and mode a2, respectively, N¯ can be interpreted as the mean number of photon pairs. As it can be seen in equation (35), the term that contains ε represents the contribution from the external driving coherent light of the parametric amplifier to the total mean photon number. Therefore, it is easy to verify that equation (35) represents the mean number of photon pairs of the system.It is not difficult to see from Figure10 that the mean number of photon pairs increases with the linear gain coefficient for κ=0.8, ε=0.399, n¯th=0.15 and for smaller values of η, but it decreases for larger values. Moreover, Figure 11 clearly indicates that the mean photon number of the cavity modes increases with the amplitude of the coherent driving light ε. In order to clearly see by what extent the coherent fields enhance the mean photon number over the laser system, we plotted in Figure 12 the mean number of photon pairs versus ε and A for η=0.1, κ=0.8, and n¯th=0.15. It is quite interesting to note from this figure that the coherent fields enhance the mean photon number over the laser system by several hundreds of mean photon numbers. Therefore, the increase in the mean photon number is observed in a region where the degree of two-mode squeezing and entanglement is significant making the system under consideration a viable source of intense squeezed as well as entangled light. We hence note that coupling the cavity to the thermal reservoir increases the mean number of photon pairs, which we believe is an encouraging result.Figure 10
Plots of the mean number of photon pairs (equation (35)) versus η for κ=0.8, ε=0.399, n¯th=0.15 and for different values of linear gain coefficients.Figure 11
Plots of the mean number of photon pairs (equation (35)) versus η for A=10, κ=0.8, n¯th=0.15 and for different values of ε.Figure 12
A plot of the mean number of photon pairs (equation (35)) versus ε and A for η=0.1, κ=0.8, and n¯th=0.15.The result presented in Figure13 indicates that the mean number of photon pairs increases with the mean photon number of the thermal reservoir at the minimum atomic coherence η. The maximum possible value of the mean number of photon pairs in this case occurs for n¯th=0.30 and small η=0. This is readily understandable since traversing more thermal mean photon number n¯th across the cavity leads to the generation of more photons. We set ε=0 so that the dependence of the mean photon number on the parameter n¯th is clearly evident from the figure.Figure 13
Plots of the mean number of photon pairs (equation (35)) versus η for A=100, κ=0.8, ε=0.0 and for different values of n¯th=0.15.


### 5.2. Mandel’sQ-Factor

It is a common experience that a nonclassical photon number correlation can be studied applying the measure of the departure of the photon statistics from the Poisson character. This measure of departure can be represented by Mandel’sQ-factor defined as(36)Q=Δn^2−n^n^,where n^=c^†c^ is the photon number operator of a two-mode cavity radiation. It is not difficult to verify that equation (36) can be expressed by putting the operators in the normal ordering as(37)Q=c^†2c^2+c^†c^2c^†c^,where c^=1/2a^1+a^2 is the annihilation operator that describes the two-mode cavity radiation. With the help of this, the normal ordering of the operators would not be altered since a^1 and a^2 commute. Hence, it is possible to put the resulting expression in terms of c-number variables associated with the normal order as(38)Q=γ∗2tγ2t+γ∗tγt2γ∗tγt,where γ=1/2α1t+α2t. Hence, employing equations (17) and (18), one obtains(39)Q=N¯+α1tα2t2N¯.It is well known that the negativity of Mandel’s parameter refers to a sub-Poissonian character of the photon statistics that essentially refers to a nonclassical property. Since the mean number of photon pairs andα1tα2t2 are positive, Mandel’s Q-factor in this case is definitely greater than 0. This ensures that the generated radiation demonstrates super-Poissonian photon statistics while exhibiting nonclassical properties such as squeezing and entanglement.Figure14 shows Mandel’s Q-factor described by equation (39) versus ε and η for A=100, κ=0.8, and n¯th=0.15. This figure indicates that Mandel’s Q-factor for the given system is definitely positive. This implies that the generated laser light demonstrates super-Poissonian photon statistics. From this plot, we see that Mandel’s Q-factor increased with the parametric amplifier at the minimum atomic coherence η, which is the maximum squeezing occurring point.Figure 14
A plot of Mandel’sQ-factor (equation (39)) versus ε and η for A=100, κ=0.8, and n¯th=0.15.The result presented in Figure15 indicates that Mandel’s Q-factor increases with the decreasing value of the atomic coherence η and with increasing the mean photon number of the thermal light n¯th. However, Figure 16 shows a plot of Mandel’s Q-factor of equation (39) versus ε and A for η=0.1, κ=0.8, and n¯th=0.15. The result in this figure indicates that the linear gain coefficient (rate of atomic injection) increases the values of Mandel’s Q-factor with at the maximum atomic coherence η. In these two figures, we observe that the value of Mandel’s Q-factor is positive.Figure 15
Plots of Mandel’sQ-factor (equation (39)) versus η for A=100, κ=0.8, ε=0.399 and for different values of n¯th.Figure 16
A plot of Mandel’sQ-factor (equation (39)) versus ε and A for η=0.1, κ=0.8, and n¯th=0.15.Moreover, as it can be described in Figure17, the value of Mandel’s Q-factor enhanced with the amplitude of the coherent light ε. Therefore, in these two figures, we observe that both the thermal reservoir and the driving coherent light increase the value of Mandel’s Q-factor.Figure 17
Plots of Mandel’sQ-factor (equation (39)) versus η for A=10, κ=0.8, n¯th=0.15 and for different values of ε.


### 5.3. Photon Number Correlations

The normalized second-order correlation function for the two-mode light can be expressed as [39](40)ga1,a220=a^1†a^2†a^1a^2a^1†a^1a^2†a^2.We realize that the operators in (39) are in the normal order. Therefore, the second-order correlation function can be expressed in terms of the c-number variables associated with the normal ordering as(41)ga1,a220=1+α1tα2t2α1∗tα1tα2∗tα2t.We plot, in Figure18, the second-order correlation function of the two-mode light versus η for A=100, κ=0.8, and ε=0.399 in the presence and absence of the thermal light n¯th. We easily see from this figure that ga1,a220 increases with η in both cases.Figure 18
Plots of the normalized second-order correlation function (equation (41)) versus η for A=100, κ=0.8, ε=0.399 and for different values of n¯th.On the other hand, the plots in Figure19 indicate that the parametric oscillator decreases the second-order correlation function for the same value of η. As this function deals with the correlation between the photon numbers, as already seen in the plots, it would not be a direct measure of the squeezing as well as entanglement of the given system.Figure 19
Plots of the normalized second-order correlation function (equation (41)) versus η for A=100, κ=0.8, n¯th=0.15 and for different values of ε.Figure20 shows the plots of the linear gain coefficient described by equation (41) versus η and A=100 for κ=0.8, ε=0.399, and n¯th=0.15. It is not difficult to see from this figure that the normalized second-order correlation function increases significantly with the linear gain coefficient and the atomic coherence η. From this, we conclude that the normalized second-order correlation of two-mode generated light increases as the degree of squeezing increases in general. Moreover, the presence of the parametric oscillator enhances the intermode correlation over the system.Figure 20
A plot of the normalized second-order correlation function (equation (41)) versus η and A=100 for κ=0.8, ε=0.399, and n¯th=0.15.


## 5.1. Mean Photon Number

In order to know about the brightness of the generated light, it is necessary to study the mean number of photon pairs describing the two-mode cavity radiation that can be defined as(34)N¯=c^†tc^t.It then follows that(35)N¯=12α1∗tα1t+α2∗tα2t.Sinceα1∗tα1t and α2∗tα2t represent the mean photon numbers in mode a1 and mode a2, respectively, N¯ can be interpreted as the mean number of photon pairs. As it can be seen in equation (35), the term that contains ε represents the contribution from the external driving coherent light of the parametric amplifier to the total mean photon number. Therefore, it is easy to verify that equation (35) represents the mean number of photon pairs of the system.It is not difficult to see from Figure10 that the mean number of photon pairs increases with the linear gain coefficient for κ=0.8, ε=0.399, n¯th=0.15 and for smaller values of η, but it decreases for larger values. Moreover, Figure 11 clearly indicates that the mean photon number of the cavity modes increases with the amplitude of the coherent driving light ε. In order to clearly see by what extent the coherent fields enhance the mean photon number over the laser system, we plotted in Figure 12 the mean number of photon pairs versus ε and A for η=0.1, κ=0.8, and n¯th=0.15. It is quite interesting to note from this figure that the coherent fields enhance the mean photon number over the laser system by several hundreds of mean photon numbers. Therefore, the increase in the mean photon number is observed in a region where the degree of two-mode squeezing and entanglement is significant making the system under consideration a viable source of intense squeezed as well as entangled light. We hence note that coupling the cavity to the thermal reservoir increases the mean number of photon pairs, which we believe is an encouraging result.Figure 10
Plots of the mean number of photon pairs (equation (35)) versus η for κ=0.8, ε=0.399, n¯th=0.15 and for different values of linear gain coefficients.Figure 11
Plots of the mean number of photon pairs (equation (35)) versus η for A=10, κ=0.8, n¯th=0.15 and for different values of ε.Figure 12
A plot of the mean number of photon pairs (equation (35)) versus ε and A for η=0.1, κ=0.8, and n¯th=0.15.The result presented in Figure13 indicates that the mean number of photon pairs increases with the mean photon number of the thermal reservoir at the minimum atomic coherence η. The maximum possible value of the mean number of photon pairs in this case occurs for n¯th=0.30 and small η=0. This is readily understandable since traversing more thermal mean photon number n¯th across the cavity leads to the generation of more photons. We set ε=0 so that the dependence of the mean photon number on the parameter n¯th is clearly evident from the figure.Figure 13
Plots of the mean number of photon pairs (equation (35)) versus η for A=100, κ=0.8, ε=0.0 and for different values of n¯th=0.15.


## 5.2. Mandel’sQ-Factor

It is a common experience that a nonclassical photon number correlation can be studied applying the measure of the departure of the photon statistics from the Poisson character. This measure of departure can be represented by Mandel’sQ-factor defined as(36)Q=Δn^2−n^n^,where n^=c^†c^ is the photon number operator of a two-mode cavity radiation. It is not difficult to verify that equation (36) can be expressed by putting the operators in the normal ordering as(37)Q=c^†2c^2+c^†c^2c^†c^,where c^=1/2a^1+a^2 is the annihilation operator that describes the two-mode cavity radiation. With the help of this, the normal ordering of the operators would not be altered since a^1 and a^2 commute. Hence, it is possible to put the resulting expression in terms of c-number variables associated with the normal order as(38)Q=γ∗2tγ2t+γ∗tγt2γ∗tγt,where γ=1/2α1t+α2t. Hence, employing equations (17) and (18), one obtains(39)Q=N¯+α1tα2t2N¯.It is well known that the negativity of Mandel’s parameter refers to a sub-Poissonian character of the photon statistics that essentially refers to a nonclassical property. Since the mean number of photon pairs andα1tα2t2 are positive, Mandel’s Q-factor in this case is definitely greater than 0. This ensures that the generated radiation demonstrates super-Poissonian photon statistics while exhibiting nonclassical properties such as squeezing and entanglement.Figure14 shows Mandel’s Q-factor described by equation (39) versus ε and η for A=100, κ=0.8, and n¯th=0.15. This figure indicates that Mandel’s Q-factor for the given system is definitely positive. This implies that the generated laser light demonstrates super-Poissonian photon statistics. From this plot, we see that Mandel’s Q-factor increased with the parametric amplifier at the minimum atomic coherence η, which is the maximum squeezing occurring point.Figure 14
A plot of Mandel’sQ-factor (equation (39)) versus ε and η for A=100, κ=0.8, and n¯th=0.15.The result presented in Figure15 indicates that Mandel’s Q-factor increases with the decreasing value of the atomic coherence η and with increasing the mean photon number of the thermal light n¯th. However, Figure 16 shows a plot of Mandel’s Q-factor of equation (39) versus ε and A for η=0.1, κ=0.8, and n¯th=0.15. The result in this figure indicates that the linear gain coefficient (rate of atomic injection) increases the values of Mandel’s Q-factor with at the maximum atomic coherence η. In these two figures, we observe that the value of Mandel’s Q-factor is positive.Figure 15
Plots of Mandel’sQ-factor (equation (39)) versus η for A=100, κ=0.8, ε=0.399 and for different values of n¯th.Figure 16
A plot of Mandel’sQ-factor (equation (39)) versus ε and A for η=0.1, κ=0.8, and n¯th=0.15.Moreover, as it can be described in Figure17, the value of Mandel’s Q-factor enhanced with the amplitude of the coherent light ε. Therefore, in these two figures, we observe that both the thermal reservoir and the driving coherent light increase the value of Mandel’s Q-factor.Figure 17
Plots of Mandel’sQ-factor (equation (39)) versus η for A=10, κ=0.8, n¯th=0.15 and for different values of ε.


## 5.3. Photon Number Correlations

The normalized second-order correlation function for the two-mode light can be expressed as [39](40)ga1,a220=a^1†a^2†a^1a^2a^1†a^1a^2†a^2.We realize that the operators in (39) are in the normal order. Therefore, the second-order correlation function can be expressed in terms of the c-number variables associated with the normal ordering as(41)ga1,a220=1+α1tα2t2α1∗tα1tα2∗tα2t.We plot, in Figure18, the second-order correlation function of the two-mode light versus η for A=100, κ=0.8, and ε=0.399 in the presence and absence of the thermal light n¯th. We easily see from this figure that ga1,a220 increases with η in both cases.Figure 18
Plots of the normalized second-order correlation function (equation (41)) versus η for A=100, κ=0.8, ε=0.399 and for different values of n¯th.On the other hand, the plots in Figure19 indicate that the parametric oscillator decreases the second-order correlation function for the same value of η. As this function deals with the correlation between the photon numbers, as already seen in the plots, it would not be a direct measure of the squeezing as well as entanglement of the given system.Figure 19
Plots of the normalized second-order correlation function (equation (41)) versus η for A=100, κ=0.8, n¯th=0.15 and for different values of ε.Figure20 shows the plots of the linear gain coefficient described by equation (41) versus η and A=100 for κ=0.8, ε=0.399, and n¯th=0.15. It is not difficult to see from this figure that the normalized second-order correlation function increases significantly with the linear gain coefficient and the atomic coherence η. From this, we conclude that the normalized second-order correlation of two-mode generated light increases as the degree of squeezing increases in general. Moreover, the presence of the parametric oscillator enhances the intermode correlation over the system.Figure 20
A plot of the normalized second-order correlation function (equation (41)) versus η and A=100 for κ=0.8, ε=0.399, and n¯th=0.15.


## 6. Conclusion

In this paper, we have studied the steady-state two-mode squeezing and entanglement of the light produced by a nondegenerate three-level cascade laser with a coherently driven parametric amplifier and coupled to a two-mode thermal reservoir in the linear and adiabatic approximation schemes in the good cavity limit. Here. we have considered a nondegenerate three-level laser in which the pump mode emerging from the parametric amplifier does not couple the top and bottom levels of the injected atoms [17]. This could be realized by putting on the right-side of the nonlinear crystal a screen which absorbs the pump mode. Moreover, we carry out our analysis by applying the master equation describing the dynamics of the optical system. Employing the solutions for c-number cavity mode variables along with the correlation property of noise forces associated with normal ordering, we obtained quadrature squeezing, the photon entanglement, the mean number of photon pairs, Mandel’s Q-factor, and the second-order correlation functions of the two-cavity light.It is found that the two-mode cavity radiation exhibits squeezing properties under certain conditions pertaining to the injected atomic coherence, where the degree of squeezing increases with the linear gain coefficient and the amplitude of the driving coherent lightε. However, the linear correlation coefficient increases with the degree of squeezing. But as the thermal light increases, the squeezing decreases. Moreover, we have found that the parametric amplifier produces a considerable degree of entangled light for a very small value of the linear gain coefficient regardless of how atoms are initially prepared. Generally, we have found that the degree of entanglement for the two-mode cavity light is directly related to the two-mode squeezing. Whenever there is squeezing in the two-mode light, there exists entanglement in the system. Since the parametric amplifier introduces additional squeezing to the system, the degree of entanglement has been enhanced for the given system. We have showed that the normalized second-order correlation of two-mode generated light increases as the degree of squeezing increases in general. Moreover, the presence of the parametric oscillator enhances the correlation of the two cavity light modes over the system. Finally, the quantum discords as a quantum correlation property can be investigated in the future.



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