# Nonclassical Effects of Light in Fifth Harmonic Generation up to First-Order Hamiltonian Interaction

Authors: Rajendra Pratap; D. K. Giri; Ajay Prasad
Journal: ISRN Optics
 (2014)

---

## Abstract

The nonclassical effects of light in the fifth harmonic generation are investigated by quantum mechanically up to the first-order Hamiltonian interaction. The coupled Heisenberg equations of motion involving real and imaginary parts of the quadrature operators are established. The occurrence of amplitude squeezing effects in both quadratures of the radiation field in the fundamental mode is investigated and found to be dependent on the selective phase values of the field amplitude. The photon statistics in the fundamental mode have also been investigated and found to be sub-Poissonian in nature. It is observed that there is no possibility to produce squeezed light in the harmonic mode up to first-order Hamiltonian interaction. Further, we have found that the normal squeezing in the harmonic mode directly depends upon the fifth power of the field amplitude of the initial pump field up to second-order Hamiltonian interaction. This gives a method of converting higher-order squeezing in the fundamental mode into normal squeezing in the harmonic mode and vice versa. The analytic expression of fifth-order squeezing of the fundamental mode in the fifth harmonic generation is established.


---

## Body

## 1. Introduction

The nonclassical effects like squeezing and sub-Poissonian photon statistics of light [1–3], which is a purely quantum mechanical phenomenon [4–6], have attracted considerable attention owing to its low-noise property [7–9] with applications in high quality telecommunication [10], quantum cryptography [11, 12], and so forth. Squeezing has been either experimentally observed or theoretically predicted in a variety of nonlinear optical processes, such as harmonic generation [13, 14], multiwave mixing processes [15–18], Raman [19–21], and hyper-Raman [22]. Hong and Mandel [23, 24], Hillery [25–27], and Zhan [28] have introduced the notion of amplitude squeezing of the quantized electromagnetic field in various nonlinear optical processes. Squeezing and photon statistical effect of the field amplitude in optical parametric and in Raman and hyper-Raman scattering processes have also been reported by Peěrina et al. [29]. Higher-order sub-Poissonian photon statistical of light have also been studied by Kim and Yoon [30]. Recently, Prakash and Mishra [31, 32] have reported the higher-order sub-Poissonian photon statistics and their use in detection of higher-order squeezing. Furthermore, higher-order amplitude squeezing with dependence on photon number in fourth and fifth harmonic generation has also been investigated by Gill et al. [33]. The nonclassical phenomena squeezing of radiation and photon statistics effects are expected to manifest itself in optical processes in which the nonlinear response of the system to the radiation field plays a great role. It also represents a new type of quantum state of the electromagnetic field and it has always been of interest to the research community in the fields of quantum optics, nonlinear optics, atomic physics, molecular physics, and biological physics; hence their study can be expected to lead to new fundamental insights.The objective of this paper is to study nonclassical effects of the light in the fundamental mode including harmonic mode in fifth harmonic generation process under short-time approximation based on a fully quantum mechanical approach up to first order Hamiltonian interaction ing
t. The paper is organized as follows. Section 2 gives the definition of squeezing and sub-Poissonian states of light. We establish the analytic expression of selective phase angle dependent amplitude squeezing and sub-Poissonian light in the fundamental mode up to first order in g
t in Section 3. The photon statistics of the pump mode in this process have also been incorporated in this section and found to be sub-Poissonian in nature. In Section 4, we study the occurrence of amplitude squeezing effects in both quadratures of the radiation field in the harmonic mode and they were found to be dependent on fifth-order squeezing of the fundamental mode. Finally, we conclude the paper in Section 5.


## 2. Definition of Nonclassical States of Light

Squeezed states of light are characterized by reduced quantum fluctuations in one quadrature of the field at the expense of the increased fluctuations in the other quadrature. It is possible to characterize the amplitude by its real and imaginary parts as(1)
X
1
=
1
2
(
A
+
A
†
)
,
X
2
=
1
2
i
(
A
-
A
†
)
,
where A
≡
A
(
t
) and A
†
≡
A
†
(
t
) are the slowly varying operators because the interaction between modes, it induces a slower dependence on time as compared to fast variation of a
(
t
)
∝
exp
⁡
(
-
i
ω
t
) and a
†
(
t
)
∝
exp
⁡
(
i
ω
t
) that are useful in discussing squeezing effects [34, 35]. For a single mode of the electromagnetic field with frequency ω and creation (annihilation) operators a
†
(
a
), the slowly varying operators defined by
(2)
A
(
t
)
=
a
(
t
)
exp
⁡
(
i
ω
t
)
,
A
†
(
t
)
=
a
†
(
t
)
exp
⁡
(
-
i
ω
t
)
.
The operators defined by (1) do not commute and obey the commutation relation
(3)
[
X
1
,
X
2
]
=
i
2
,
and, as a result, they satisfy the uncertainty relation (ħ= 1)
(4)
Δ
X
1
Δ
X
2
≥
1
4
,
where Δ
X
1 and Δ
X
2 are the uncertainties in the quadrature operators X
1 and X
2, respectively. A quantum state is squeezed in the X
1 direction if Δ
X
1
<
1
/
2 and is squeezed in the X
2 direction if Δ
X
2
<
1
/
2.In order to define higher-order squeezing i.e. amplitude squared squeezing [25, 26], we represent the real and imaginary parts of the square of the field amplitude in terms of operators Y
1 and Y
2 as
(5)
Y
1
=
1
2
(
A
2
+
A
†
2
)
,
Y
2
=
1
2
i
(
A
2
-
A
†
2
)
.
The operators defined by (5) do not commute and obey the commutation relation
(6)
[
Y
1
,
Y
2
]
=
i
(
2
N
A
+
1
)
.
The commutation relation of (6) leads to the uncertainty relation
(7)
Δ
Y
1
Δ
Y
2
≥
〈
(
N
A
+
1
2
)
〉
,
where Δ
Y
1 and Δ
Y
2 are the uncertainties in the quadrature operators Y
1 and Y
2, respectively. A quantum state is squeezed in the Y
1 direction if (
Δ
Y
1
)
2
<
〈
(
N
A
+
1
/
2
)
〉 and is squeezed in the Y
2 direction if (
Δ
Y
2
)
2
<
〈
(
N
A
+
1
/
2
)
〉.Similarly, it is possible to characterize the fifth power of the field amplitude [22] by its real and imaginary parts as
(8)
G
1
=
1
2
(
A
5
+
A
†
5
)
,
G
2
=
1
2
i
(
A
5
-
A
†
5
)
.
The operators defined by (8) do not commute and obey the commutation relation
(9)
[
G
1
,
G
2
]
=
i
2
(
25
N
A
4
+
50
N
A
3
+
275
N
A
2
+
250
N
A
+
120
)
=
i
2
(
G
{
12
}
)
,
where we introduce the auxiliary function (
G
{
12
}
) instead of (
25
N
A
4
+
50
N
A
3
+
275
N
A
2
+
250
N
A
+
120
).And the commutation relation of (9) follows the uncertainty relation as
(10)
Δ
G
1
Δ
G
2
≥
1
4
〈
(
G
{
12
}
)
〉
.
Hence the fifth-order squeezing is said to exist if
(11)
(
Δ
G
1
)
2
or
(
Δ
G
2
)
2
<
1
4
〈
(
G
{
12
}
)
〉
.
The quantum effect of sub-Poissonian photon statistics is the reduction of quantum fluctuations in photon number which is reflected by an increase of fluctuations of phase of the field. Hence the photon number uncertainty [36] is
(12)
〈
(
Δ
N
A
)
2
〉
<
〈
N
A
〉
.


## 3. Nonclassical Effects of Light in the Fundamental Mode

Fifth harmonic generation is a process in which an incident laser beam of the fundamental frequencyω
1 interacts with a nonlinear medium to produce the harmonic frequency at ω
2
=
5
ω
1.The present model, shown in Figure1, has been adopted from the works of Chang et al. [37] who have studied the optimal combination of nonlinear optical crystals for the fifth harmonic generation and Ni et al. [38] have reported the comparative experimental investigation on third and fifth harmonic generation by mid-infrared ultrafast laser pulses. This model is chosen to make a realistic one and our discussions hold for all similar models.Figure 1
Fifth harmonic generation energy level model.In this model (Figure1), the interaction is looked upon as a process involving absorption of five pump photons of frequency ω
1 each and the system going from state |
1
〉 to state |
2
〉 and emission of one photon of frequency ω
2 and the atomic system is finally coming back to the initial state |
1
〉.The Hamiltonian for this process can be written as (ħ = 1)
(13)
H
=
ω
1
a
†
a
+
ω
2
b
†
b
+
g
(
a
5
b
†
+
a
†
5
b
)
,wherea
†
(
a
) and b
†
(
b
) are the creation (annihilation) operators of the pump field (A-mode) and harmonic field (B-mode), respectively, and g is the coupling constant in the interaction Hamiltonian, which is assumed to be real, describes the coupling between the two modes of the order of 102–104 per second and is proportional to the nonlinear susceptibility of the medium as well as the complex amplitude of the pump field [39, 40]. However, to take care of complex g, we have used |
g
|
2 in the place of g
2 as we are not considering the phase terms. In the case of phase matching, g can also be treated as real [4]. Furthermore, in an earlier publication [41], it is shown that the real part of g plays an important role in the generalization of squeezed light.Since the time dependence of free modes(
g
=
0
) is simply proportional to exp
⁡
(
i
ω
1
t
) or exp
⁡
(
i
ω
2
t
). The interaction between modes (
g
≠
0
) induces a slower dependence on time and we can write A
(
t
)
=
a
(
t
)
exp
⁡
(
i
ω
1
t
) and B
(
t
)
=
b
(
t
)
exp
⁡
(
i
ω
2
t
) with the relation ω
2
=
5
ω
1, where the operators A
(
t
) and B
(
t
) vary slowly in time. Later it will be evident that A
(
t
) and B
(
t
) indeed depend on a scaled time “g
t” (not on t), thus satisfying their slow variation of the operators A
(
t
) and B
(
t
) as compared to fast variation of a
(
t
) and b
(
t
) since g
≪
ω
1, ω
2 usually.Using the Hamiltonian interaction of (13) in the coupled Heisenberg equation of motion, we have
(14)
A
˙
(
t
)
=
∂
A
(
t
)
∂
t
+
i
[
H
,
A
(
t
)
]
(
ħ
=
1
)
,
where the dot denotes time derivative and the partial time derivative term and Hamiltonian interaction in Heisenberg picture is represented as
(15)
∂
A
(
t
)
∂
t
=
i
ω
1
a
(
t
)
exp
⁡
(
i
ω
1
t
)
=
i
ω
1
A
(
t
)
,
i
[
H
,
A
(
t
)
]
=
-
i
ω
1
A
(
t
)
-
5
i
g
t
A
†
4
(
t
)
B
(
t
)
.
Using the values in (14), we obtain Heisenberg’s equations of motion for the slowly varying amplitude operator A
(
t
) up to the first-time derivative [25, 28] as
(16)
A
˙
(
t
)
=
-
5
i
g
A
†
4
(
t
)
B
(
t
)
.
Similarly, we have
(17)
B
˙
(
t
)
=
-
i
g
A
5
(
t
)
.
Since the general time-dependent solution of the set of coupled differential equations (16) and (17) is not available, let us approximately solve them in the short-time limit. Note that the system evolution during a short period of time is practically relevant because the actual interaction is in fact very short. Hence the interaction time is taken to be short and to be of the order of 10−10 sec and a nanosecond or picosecond pulse laser can be used as the pump field. For real physical situation in the short-time scale g
t
≪
1
(
g
t
~
10
-
6
) and when the number of photons is very large (
|
α
|
2
≫
1
), it is possible to obtain much simpler approximate analytical formulas describing the variances. Expanding A
(
t
) around the initial time t
=
0 in Taylor’s expansion [28] and confining ourselves to terms up tofirst order in “
t
,” we have
(18)
A
(
t
)
=
A
(
0
)
+
t
A
˙
(
0
)
+
⋯

.
In (18) the operators A
(
0
)
≡
A and A
˙
(
0
)
≡
(
∂
A
(
t
)
/
∂
t
)
|
t
=
0 without an argument are opeators evaluated at t
=
0. This convention is followed throughout the paper.Using (16) in (18), we obtain up tofirst order in “
g
t
”
(19)
A
(
t
)
=
A
(
0
)
-
5
i
g
t
A
†
4
(
0
)
B
(
0
)
=
A
-
5
i
g
t
A
†
4
B
.
Equation (19) indicates that A
(
t
) depends on g
t rather than on t revealing the much slower variation of A
(
t
) as compared to the fast variation of a
(
t
).Then in reversal order,(20)
A
†
(
t
)
=
A
†
+
5
i
g
t
A
4
B
†
.
Similarly,
(21)
B
(
t
)
=
B
-
i
g
t
A
5
,
B
†
(
t
)
=
B
†
+
i
g
t
A
†
5
.In order to examine the amplitude squeezing of the fundamental modeA, as a function of time, we define quadrature components by
(22)
X
1
A
(
t
)
=
1
2
[
A
(
t
)
+
A
†
(
t
)
]
,
X
2
A
(
t
)
=
1
2
i
[
A
(
t
)
-
A
†
(
t
)
]
.
Using (19) and (20) in (22), we obtain
(23)
X
1
A
(
t
)
=
1
2
[
(
A
+
A
†
)
-
5
i
g
t
(
A
†
4
B
-
A
4
B
†
)
]
,
(24)
X
2
A
(
t
)
=
1
2
i
[
(
A
-
A
†
)
-
5
i
g
t
(
A
†
4
B
+
A
4
B
†
)
]
.Now, we assume an initial quantum state as a product of coherent states|
α

> for the fundamental mode A and |
β

> for the harmonic mode B; that is,
(25)
|
ψ


>
=
|
α
>
A
|
β
>
B
.
Using (25) in (23), we obtain the expectation value as
(26)
〈
ψ
|
X
1
A
2
(
t
)
|
ψ
〉
=
1
4
[
α
2
+
α
*
2
+
2
|
α
|
2
+
1
-
10
i
g
t
d
d
×
(
|
α
|
2
α
*
3
β
+
2
α
*
3
β
-
2
α
3
β
*
c
d
d
d
d
-
|
α
|
2
α
3
β
*
+
α
*
5
β
-
α
5
β
*
)
]
,
〈
ψ
|
X
1
A
(
t
)
|
ψ
〉
2
=
1
4
[
α
2
+
α
*
2
+
2
|
α
|
2
-
10
i
g
t
d
d
×
(
|
α
|
2
α
*
3
β
+
α
*
5
β
-
α
5
β
*
d
d
d
d
d
-
|
α
|
2
α
3
β
*
)
]
.
Hence, the field variance is
(27)
[
Δ
X
1
A
(
t
)
]
2
=
〈
X
1
A
2
(
t
)
〉
-
〈
X
1
A
(
t
)
〉
2
=
1
4
[
1
-
10
i
g
t
(
2
α
*
3
β
-
2
α
3
β
*
)
]
.
Equations (4) and (27) yield
(28)
[
Δ
X
1
A
(
t
)
]
2
-
1
4
=
10
|
g
t
|
|
α
3
β
|
sin
(
θ
2
-
3
θ
1
)
,
where 〈
N
A
〉
=
〈
A
†
A
〉
=
|
α
|
2 and 〈
N
B
〉
=
〈
B
†
B
〉
=
|
β
|
2 are the photon number operators in the modes A and B, respectively, and α
=
|
α
|
exp
⁡
(
i
θ
1
) and β
=
|
β
|
exp
⁡
(
i
θ
2
) are dimensionless complex numbers; θ
1 and θ
2 are the phase angles; α
*, β
* denote the complex conjugate of α and β, respectively. From (28) it is found that the squeezing of X
1
A will occur whenever sin
(
θ
2
-
3
θ
1
)
<
0.Similarly, using (24) and (25) for X
2
A direction, we have
(29)
[
Δ
X
2
A
(
t
)
]
2
-
1
4
=
-
10
|
g
t
|
|
α
3
β
|
sin
(
θ
2
-
3
θ
1
)
.
The right-hand side of (29) is negative when sin
(
θ
2
-
3
θ
1
)
>
0, showing the existence of normal squeezing in the fundamental mode up to first order in g
t in the fifth harmonic generation process. Equations (28) and (29) show that only one quadrature can be squeezed at a time; that is, it follows Heisenberg’s uncertainty principle.To measure the degree of amplitude squeezing, we define the normalized parameter [30] of (29) as
(30)
Q
x
=
[
Δ
X
2
A
(
t
)
]
2
-
1
/
4
1
/
4
=
-
40
|
g
t
|
|
α
3
β
|
sin
(
θ
2
-
3
θ
1
)
.
Hence the degree of amplitude squeezing of the fundamental mode is found to be dependent directly on the phase angle of the field amplitude up to the first-order Hamiltonian interaction in g
t.We plot a graph of (30) between the normalized parameter of squeezing Q
x and the photon number |
α
|
2 with different values of |
β
| in Figure 2.Figure 2
Dependence of degree of normal squeezingQ
x with |
α
|
2and |
β
| in fifth harmonic generation (when |
g
t
|
=
1
0
-
4 and θ
1
=
0 and θ
2
=
π
/
2
).Figure2 shows that the normal squeezing increases nonlinearly with the increase the value of |
α
|
2. We observe that when higher the value of |
β
|, then the squeezing increases and it lowers the depth of classicality of the field amplitude. It shows that the degree of normal squeezing depends directly upon the photon number of the fundamental mode as well as of the harmonic mode.Similarly for studying one of the class of higher-order squeezing like squeezing of amplitude-squared of the field of the fundamental mode as a function of time, we define quadrature components for the pump mode as(31)
Y
1
A
(
t
)
=
1
2
[
A
2
(
t
)
+
A
†
2
(
t
)
]
,
(32)
Y
2
A
(
t
)
=
1
2
i
[
A
2
(
t
)
-
A
†
2
(
t
)
]
.
Using (19) and (20) in (31), we get
(33)
Y
1
A
(
t
)
=
1
2
[
A
2
+
A
†
2
-
10
i
g
t
d
d
×
(
A
†
4
A
B
+
2
A
†
3
B
-
A
†
A
4
B
†
-
2
A
3
B
†
)
]
.
Using (25) in (33), we obtain the expectation value as
(34)
〈
ψ
|
Y
1
A
2
(
t
)
|
ψ
〉
=
1
4
[
α
4
+
α
*
4
+
2
|
α
|
4
+
4
|
α
|
2
+
2
d
d
d
.
d
d
.
-
20
i
g
t
(
|
α
|
6
α
*
β
-
|
α
|
6
α
β
*
+
6
|
α
|
4
α
*
β
d
d
d
d
d
.
d
d
d
d
d
d
d
d
.
-
6
|
α
|
4
α
β
*
+
12
|
α
|
2
α
*
β
-
12
|
α
|
2
α
β
*
d
d
d
d
d
.
d
d
d
d
d
d
d
d
.
+
|
α
|
2
α
*
5
β
-
|
α
|
2
α
5
β
*
+
3
α
*
5
β
-
3
α
5
β
*
d
d
d
d
d
.
d
d
d
d
d
d
d
d
.
+
6
α
*
β
-
6
α
α
*
)
2
|
α
|
4
]
,
〈
ψ
|
Y
1
A
(
t
)
|
ψ
〉
2
=
1
4
[
α
4
+
α
*
4
+
2
|
α
|
4
-
20
i
g
t
d
d
d
d
d
×
(
2
|
α
|
4
α
*
β
-
2
|
α
|
4
α
β
*
+
|
α
|
6
α
*
β
-
|
α
|
6
α
β
*
d
d
d
d
d
d
d
d
+
|
α
|
2
α
*
5
β
-
|
α
|
2
α
5
β
*
+
2
α
*
5
β
-
2
α
5
β
*
)
]
.
And the expectation value of the time-dependent mean photon number is
(35)
〈
N
A
(
t
)
〉
=
|
α
|
2
-
5
i
g
t
(
α
*
5
β
-
α
5
β
*
)
.
Using (34)-(35) in (7), we get
(36)
[
Δ
Y
1
A
(
t
)
]
2
-
〈
N
A
(
t
)
+
1
/
2
〉
=
40
|
g
t
|
|
α
β
|
sin
(
-
θ
1
+
θ
2
)
×
{
(
|
α
|
4
+
3
|
α
|
2
+
3
/
2
)
}
.
Similarly, we get for Y
2
A quadrature
(37)
[
Δ
Y
2
A
(
t
)
]
2
-
〈
N
A
(
t
)
+
1
/
2
〉
=
-
40
|
g
t
|
|
α
β
|
sin
(
-
θ
1
+
θ
2
)
×
{
(
|
α
|
4
+
3
|
α
|
2
+
3
/
2
)
}
.
The right-hand sides of (36) and (37) are showing the existence of squeezing in amplitude-squared of the field in the fundamental mode in the fifth harmonic generation process whenever sin
(
-
θ
1
+
θ
2
)
<
0 and sin
(
-
θ
1
+
θ
2
)
>
0, respectively. The multiplication factor (
|
α
|
4
+
3
|
α
|
2
+
3
/
2
) is the nonlinear effect due to strong pump field interaction.Now, we define the normalized parameter [30] for amplitude-squared squeezing as
(38)
Q
y
=
[
Δ
Y
2
A
(
t
)
]
2
-
〈
(
N
A
(
t
)
+
1
/
2
)
〉
〈
(
N
A
(
t
)
+
1
/
2
)
〉
=
-
40
|
g
t
|
|
α
β
|
sin
(
-
θ
1
+
θ
2
)
{
(
|
α
|
4
+
3
|
α
|
2
+
3
/
2
)
}
(
|
α
|
2
+
1
/
2
)
+
10
|
g
t
|
|
α
5
β
|
sin
(
θ
2
-
5
θ
1
)
.
Hence the degree of amplitude-squared (second order) squeezing in the fundamental mode depends directly upon the phase angle of the field amplitude up to the first-order Hamiltonian interaction in g
t. The variation of Q
y with |
α
|
2 is shown in Figure 3.Figure 3
Dependence of degree of higher-order (amplitude-squared) squeezingQ
y with |
α
|
2 and |
β
| in fifth harmonic generation (when |
g
t
|
=
1
0
-
4 and θ
1
=
0 and θ
2
=
π
/
2).In Figure3, the steady fall of the curve shows that the squeezing increases nonlinearly with |
α
|
2, which depends directly upon the number of photons. This confirms that the reduction of quantum noise is associated with a large number of photons. We also find that when higher the value of |
β
|, then the squeezing increases and it lowers the depth of classicality of the field amplitude. It confirms that the degree of squeezing depends directly upon the photon number of the fundamental as well as of the harmonic field.A comparison between Figures2 and 3 shows greater noise reduction in higher order; that is, squeezing is maximum in amplitude-squared of the field (second order) than the first order having the same number of photons. Since higher-order squeezing (second order squeezing) is the higher powers of the field amplitude of the fundamental mode, which is directly associated with the large number of photons that it makes possible to achieve significantly larger signal noise reduction than the ordinary squeezing (normal or first-order squeezing).Now, using (35), we obtain expectation values of mean photon number as
(39)
〈
N
A
2
(
t
)
〉
=
|
α
|
4
+
|
α
|
2
-
5
i
g
t
×
(
2
|
α
|
2
α
*
5
β
-
2
|
α
|
2
α
5
β
*
+
5
α
*
5
β
-
5
α
5
β
*
)
,
〈
N
A
(
t
)
〉
2
=
|
α
|
4
-
5
i
g
t
(
2
|
α
|
2
α
*
5
β
-
2
|
α
|
2
α
5
β
*
)
.
Hence the fluctuation of time-dependent mean photon number is
(40)
[
Δ
N
A
(
t
)
]
2
=
〈
N
A
2
(
t
)
〉
-
〈
N
A
(
t
)
〉
2
=
|
α
|
2
-
25
i
g
t
(
α
*
5
β
-
α
5
β
*
)
,
and the photon statistics of pump mode in fifth harmonic generation is found to be sub-Poissonian, as
(41)
[
Δ
N
A
(
t
)
]
2
-
〈
N
A
(
t
)
〉
=
40
|
g
t
|
|
α
5
β
|
sin
(
θ
2
-
5
θ
1
)
.
The right-hand side of (41) is always negative whenever sin
(
-
5
θ
1
+
θ
2
)
<
0, showing the existence of sub-Poissonian light in fundamental mode up to first order Hamiltonian interaction in g
t under short-time approximation in the fifth harmonic generation process. It also indicates that the occurrence of sub-Poissonian light in the fundamental mode depends directly upon the phase angle of the field amplitude. These results are one of the distinguished examples of fifth harmonic generation process when light exhibits both squeezing and sub-Poissonian photon statistics at the same time up to first-order Hamiltonian interaction.


## 4. Nonclassical Effects of Light in the Harmonic Mode

It is of interest to examine squeezing in the harmonic modeB as a function of time; we define the quadrature operators
(42)
X
1
B
(
t
)
=
1
2
[
B
(
t
)
+
B
†
(
t
)
]
,
X
2
B
(
t
)
=
1
2
i
[
B
(
t
)
-
B
†
(
t
)
]
.
Using (21) in (42), we find
(43)
X
1
B
(
t
)
=
1
2
[
(
B
+
B
†
)
-
i
g
t
(
A
5
-
A
†
5
)
]
,
(44)
X
2
B
(
t
)
=
1
2
i
[
(
B
-
B
†
)
-
i
g
t
(
A
5
+
A
†
5
)
]
.
Using (25) in (43), we obtain
(45)
〈
ψ
|
X
1
B
2
(
t
)
|
ψ
〉
=
1
4
[
β
2
+
β
*
2
+
2
|
β
|
2
+
1
d
d
d
d
-
2
i
g
t
(
α
5
β
+
α
5
β
*
-
α
*
5
β
-
α
*
5
β
*
)
]
,
〈
ψ
|
X
1
B
(
t
)
|
ψ
〉
2
=
1
4
[
β
2
+
β
*
2
+
2
|
β
|
2
d
d
d
d
-
2
i
g
t
(
α
5
β
+
α
5
β
*
-
α
*
5
β
-
α
*
5
β
*
)
]
.
Hence
(46)
[
Δ
X
1
B
(
t
)
]
2
=
〈
X
1
B
2
(
t
)
〉
-
〈
X
1
B
(
t
)
〉
2
=
1
4
.
Similarly, from (44), we have
(47)
[
Δ
X
2
B
(
t
)
]
2
=
1
4
.
From (46) and (47), we can see that the B-mode is initially in a coherent state; that is,
(48)
[
Δ
X
1
B
]
2
=
[
Δ
X
2
B
]
2
=
1
4
.
Hence there is no possibility to produce squeezed light in the harmonic mode up to first-order Hamiltonian interaction in g
t.It is now interesting to further study squeezing in theB-mode (harmonic) up to second-order Hamiltonian interaction in g
t of the fundamental mode.From (17), we may obtain
(49)
B
¨
=
-
g
2
(
G
{
12
}
)
B
.
Using (18) and the corresponding results in the amplitude harmonic mode is up to second order in “g
t”, we get
(50)
B
(
t
)
=
B
(
0
)
-
i
g
t
A
5
-
1
2
|
g
t
|
2
(
G
{
12
}
)
B
,
B
†
(
t
)
=
B
†
(
0
)
+
i
g
t
A
†
5
-
1
2
|
g
t
|
2
(
G
{
12
}
)
B
†
.
Using (50) and (8) in (42), we get
(51)
X
1
B
(
t
)
=
X
1
B
+
g
t
G
2
A
-
1
2
|
g
t
|
2
(
G
{
12
}
)
X
1
B
,
X
2
B
(
t
)
=
X
2
B
-
g
t
G
1
A
-
1
2
|
g
t
|
2
(
G
{
12
}
)
X
2
B
.
For uncorrelated modes at t
=
0, we get the field variance in harmonic mode as
(52)
[
Δ
X
1
B
(
t
)
]
2
=
(
Δ
X
1
B
)
2
+
|
g
t
|
2
×
[
(
Δ
G
2
A
)
2
-
〈
(
G
{
12
}
)
〉
(
Δ
X
1
B
)
2
]
,
[
Δ
X
2
B
(
t
)
]
2
=
(
Δ
X
2
B
)
2
+
|
g
t
|
2
×
[
(
Δ
G
1
A
)
2
-
〈
(
G
{
12
}
)
〉
(
Δ
X
2
B
)
2
]
.
Using (48), then we have
(53)
[
Δ
X
1
B
(
t
)
]
2
-
1
4
=
|
g
|
2
t
2
[
(
Δ
G
2
A
)
2
-
1
4
〈
(
G
{
12
}
)
〉
]
,
(54)
[
Δ
X
2
B
(
t
)
]
2
-
1
4
=
|
g
|
2
t
2
[
(
Δ
G
1
A
)
2
-
1
4
〈
(
G
{
12
}
)
〉
]
.
Equations (53) and (54) show that X
1
B in the harmonic mode is squeezed if G
2
A is squeezed and X
2
B is squeezed if G
1
A is squeezed. In other words, the harmonic mode is squeezed in the X
1
B direction if the fundamental mode is fifth-order squeezing in the G
2
A direction and the harmonic mode is squeezed in the X
2
B direction if the fundamental mode is fifth-order squeezing in the G
1
A direction. That is, if a fundamental mode with fifth-order squeezing propagates through a nonlinear medium, a squeezed harmonic mode is generated.Now, comparing the results of (54) with (A.11) [see Appendix for details of the calculation of (A.11)], then we have (we consider here only the G
1
A
(
t
) quadrature)
(55)
[
Δ
X
2
B
(
t
)
]
2
-
1
4
=
-
(
5
4
)
|
g
t
|
4
×
{
(
10
|
α
|
18
+
2800
|
α
|
16
+
26400
|
α
|
14
d
d
d
d
d
d
d
+
97680
|
α
|
12
+
116880
|
α
|
10
)
cos
⁡
(
10
θ
)
d
d
d
d
d
d
+
10
|
α
|
18
+
430
|
α
|
16
+
8690
|
α
|
14
+
94343
|
α
|
12
d
d
d
d
d
d
+
514138
|
α
|
10
+
1389600
|
α
|
8
+
1756800
|
α
|
6
d
d
d
d
d
d
+
936000
|
α
|
4
+
149760
|
α
|
2
+
5760
|
α
|
12
}
.The right hand side of (55) shows that the squeezing in the harmonic mode is |
g
t
|
2 times more than the fifth-order amplitude squeezing in the fundamental mode in the fifth harmonic generation process. This establishes the fact that the occurrence of squeezing in the harmonic mode is only due to the presence of the fundamental mode. An analysis of (55) shows that if g
2
t
2
<
1, squeezing is greater in harmonic mode compared to fundamental mode. Further, a comparison between the results of (30), (38), (41) and (55) with our earlier work [42] it is observed that the squeezing and sub-Poissonian effects of light are more pronounced to reduce the quantum noise in the fifth harmonic generation than the corresponding squeezing and sub-Poissonian effects of light in the fourth harmonic generation.To study optimum squeezing in harmonic mode, we denote the right-hand side of (55) by S
X, and taking |
g
t
|
2
=
10
-
4 and θ
=
0. The variation of S
X with |
α
|
2 is shown in Figure 4.Figure 4
Dependence of harmonic squeezingS
x with |
α
|
2 in fifth harmonic generation (when |
g
t
|
2
=
1
0
-
4 and θ
=
0
).Figure4 shows that the squeezing increases nonlinearly with |
α
|
2, which is directly dependent upon the number of photons. This again confirms that the squeezed states are associated with a large number of photons. Moreover, the curve also establishes the relationship between the harmonic mode and the fundamental mode.


## 5. Conclusions

The important results of this paper can be listed as follows.
(i)
The existence of amplitude squeezing inX
1
A or X
2
A quadrature up to the first order Hamiltonian interaction in g
t in the fundamental mode will occur whenever sin
⁡
(
θ
2
-
3
θ
1
)
<
0 or sin
(
θ
2
-
3
θ
1
)
>
0 respectively. Similarly the existence of amplitude-squared i.e. second-order squeezing in Y
1
A or Y
2
A quadrature of the fundamental mode will occur whenever sin
(
-
θ
+
θ
)
<
0 or sin
-
(
θ
1
+
θ
2
)
>
0 under short-time approximation in the fifth harmonic generation process. The multiplication factor (
|
α
|
4
+
3
|
α
|
2
+
3
/
2
) in the second-order squeezing is the nonlinear effect due to strong pump field interaction.
(ii)
In the fifth harmonic generation process up to the first-order Hamiltonian interaction ing
t
, the sub-Poissonian photon statistics exists in the fundamental mode when sin
(
-
5
θ
1
+
θ
2
)
<
0.
(iii)
We have found that the degree of squeezing and sub-Poissonian photon statistics in the fundamental mode are directly dependent upon the selective phase values of the field amplitude up to the first-order interaction ing
t in the fifth harmonic generation process.
(iv)
It is observed that when higher the value of|
β
|, then squeezing increases and it lowers the depth of classicality of the field amplitude. The degree of squeezing is found to be dependent on the photon number of fundamental field as well as on the harmonic field.
(v)
There is no possibility to produce squeezed laser light in the harmonic mode up to first-order Hamiltonian interaction ing
t.
(vi)
The Hamiltonian interaction up to second order ing
t revealed that the harmonic mode is squeezed in the X
1
B direction if the fundamental mode is fifth-order squeezing in the G
2
A direction and the harmonic-mode is squeezed in the X
2
B direction if the fundamental mode is fifth-order squeezing in the G
1
A direction. That is, the squeezing in the harmonic mode depends on the fifth-order squeezing of the fundamental mode. This gives a method of converting higher-order squeezing into normal squeezing in harmonic mode.
(vii)
We have observed the fact that the occurrence of amplitude squeezing in the harmonic mode is only due to the presence of the fundamental mode.
(viii)
In an analysis of (55), it is observed that squeezing in the harmonic mode is |
g
t
|
2 times more than the fifth-order amplitude squeezing in the fundamental mode in the fifth harmonic generation process. This fact established the relationship between fundamental and harmonic mode. It is found that if g
2
t
2
<
1 squeezing is greater in harmonic mode compared to fundamental mode.
(ix)
Moreover, we have found that the squeezing increases nonlinearly with|
α
|
2, which is directly dependent upon the number of photons. This has confirmed that the squeezed states (reduction of quantum noise) are associated with a large number of photons.
(x)
One of the higher-order squeezing in fifth harmonic generation process, that is, fifth-order squeezing, is found to be more squeezed than the fourth-order squeezing [43]. Hence, the higher-order squeezing makes it possible to achieve significantly larger noise reduction than lower-order or ordinary squeezing.
(xi)
The maximum reachable degree of squeezing is directly dependent upon the short interaction time as well as the number of photons. However, the maximum attainable squeezing will be limited by short interaction time.
(xii)
It is observed that the squeezing and sub-Poissonian effects of light are more pronounced to reduce the quantum noise in the fifth harmonic generation than the corresponding squeezing and sub-Poissonian effects of light in the fourth harmonic generation [42].As a result, the family of nonclassical effects like squeezing and sub-Poissonian photon statistics in relation to selective phase values of the field amplitude up to the first-order Hamiltonian interaction in g
t are useful to obtain the desired degree of amplitude squeezing through different higher-order nonlinear optical processes. Hence, these results may pave the way for obtaining greater noise reduction in any optical systems and can be useful in high quality quantum telecommunication.



---

*Source: 580262-2014-03-09.xml*