# Field Squeezing in a Quantum-Dot Molecule Jaynes-Cummings Model

Authors: Xu Chu; Xiaodong Ma; Ying Wang; Qingchun Zhou; Yu Zhou
Journal: Advances in Optics
 (2014)

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## Abstract

We investigate the field squeezing in a system composed of an initial coherent field interacting with two quantum dots coupled by electron tunneling. An approximate quantum-dot molecule Jaynes-Cummings model describing the system is given, and the effects of physical quantities, such as the temperature, phonon-electron interaction, mean photon number, field detuning, and tunneling-level detuning, are discussed in detail.


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## Body

## 1. Introduction

Thanks to the rapid progress of nanotechnologies, the exploration of the quantum-dot system, a mesoscopic synthetic material with a quantum confinement configuration, has provided a versatile tool for the simulation of many interesting phenomena in condensed matter physics [1, 2], among which, the quantum-dot molecule (QDM), formed from an asymmetric double quantum-dot system coupled by tunneling, has attracted much attention recently. New trends in nanotechnology even enable us to manipulate this kind of QDM using the external controlment, that is, electric field or optical field.The interaction between atoms and field, an intriguing topic in modern quantum optics, yields many novel properties of the optical system. Based on the study of Jaynes-Cummings model, a fully quantum mechanical model and one of the few exactly solvable models that describes an atom in an external field, many studies have been made including the generalization of the model, such as applying the initial conditions [3], considering the dissipation and damping [4], multilevel of atoms, and multimode field [5, 6]. Many nonclassical effects have been investigated within the framework of this model, like Rabi oscillations, collapse-revival phenomenon, sub-Poissonian photon statistics, and squeezed state of the radiation field [7, 8]. Specifically, the squeezed state of light, a pure quantum effect without classical parallelism, has attracted much attention in these decades [9]; it can be widely used in the exploration of gravitational wave [10, 11], nonlinear optics [12], quantum information [13], quantum communication [14], and even precision metrology [15].For its artificial nature and properties similar to natural atoms and molecules, the QDM, an ideal candidate for the mimic of atoms interacting with external fields, has been studied extensively, because its levels could be controlled conveniently and tuned easily [16]. However, the QDM is often surrounded by the solid matrix which means that the electrons are inevitably coupled with phonons and it hints that the electron-phonon interaction cannot be neglected during the tunneling. Therefore the zero-temperature treatment is not always valid and the temperature of the environment has a significant role [17]. Although the population of all states has been analyzed, the squeezing effect of the QDM has not been investigated. In this paper we consider the squeezing of a single-mode field interacting with a QDM and study analytically and numerically how the squeezing depends on various tunable parameters of the system.This paper is arranged as follows; the next section gives the model of the external field interacting with a QDM and the equations describing the system are given; in Section3 the squeezing of the optical field is considered from different perspectives while Section 4 gives the discussion and summary.


## 2. The Model

Consider a pulsed laser field interacting with a QDM with the configuration that state|
0
〉 is the ground state without excitation while states |
1
〉 and |
2
〉 are excited states representing an electron in the left dot and one hole in the left dot [16]. For the sake of the far off-resonance of the valence band levels of two dots, other states are hardly coupled with these states; hence they are neglected here for simplicity without the loss of generality. The single-mode field with frequency ω couples the states |
0
〉 and |
1
〉 with detuning δ; states |
0
〉 and |
2
〉 are uncoupled in the time scale we consider here; quantum electronic tunneling T
e between states |
1
〉 and |
2
〉 can be controlled by voltage.Because of the low-enough temperature considered here, most of the electron-phonon interaction is the result of the deformation of the potential while the coupling constantg
k of this interaction is determined by the quantum-dot material and lattice configuration. Using the assumption that other factors causing the interaction are negligible, hence all the phonon-electron interactions can be treated as caused by the potential deformation [18]. So it is reasonable to apply the Einstein model with all the phonons having the same frequency ω
k
=
ω
0. Under the dipole approximation and the rotating-wave approximation, the Hamiltonian of the system in the interaction picture reads (
ℏ
=
1
) [19]:
(1)
H
I
=
T
e
(
R
21
e
-
i
ω
12
t
+
R
21
e
i
ω
12
t
)
e
-
S
+
λ
(
a
^
†
R
01
e
-
i
(
δ
-
Δ
)
t
+
a
^
R
10
e
i
(
δ
-
Δ
)
t
)
e
-
S
/
2
,
where Δ
=
∑
k
‍
g
k
2
/
(
4
ω
k
) and detuning δ
=
ω
10
-
ω, ω
12
=
ω
1
-
ω
2. The item representing the phonon effects, which has the expression S
=
2
∑
k
‍
(
N
+
1
/
2
)
(
g
k
/
2
ω
k
)
2 = 2
(
N
+
1
/
2
)
∑
k
‍
(
g
k
2
/
4
ω
k
2
) = 2
(
N
+
1
/
2
)
G, where G is Huang-Rhys factor expressed as ∑
k
‍
(
g
k
2
/
4
ω
k
2
) [20], corresponds to the electron-phonon interaction with temperature-dependent phonon population N
=
1
/
(
e
ω
k
/
T
-
1
). In Hamiltonian (1), R
i
j
=
|
i
〉
〈
j
|
(
i
,
j
=
0,1
,
2
) corresponds to the transition operators of the QDM, T
e is tunneling matrix element between the left and right dots, λ is the field-QDM coupling constant, and a
^
† (a
^) is the creation (annihilation) operator of the optical field satisfying [
a
^
,
a
^
†
]
=
1. In the model, both ω
12 and T
e can be manipulated by an external voltage.We suppose that initially the QDM is in the ground state|
0
〉 and the system is described as
(2)
|
ψ
(
0
)
〉
=
|
ψ
A
(
0
)
〉
⊗
|
ψ
F
(
0
)
〉
=
∑
n
=
0
∞
F
n
|
0
,
n
〉
,
where |
ψ
F
(
0
)
〉 is the arbitrary optical field, and then the state vector of the system at time t takes the form
(3)
|
ψ
(
t
)
〉
=
∑
n
‍
[
c
n
(
t
)
|
2
,
n
〉
+
b
n
(
t
)
|
1
,
n
〉
+
a
n
+
1
(
t
)
|
0
,
n
+
1
〉
]
;
hence the substitution of state vector (3) into Schrödinger’s equation yields a set of differential equations describing the expanding coefficients as
(4)
i
(
a
˙
n
+
1
b
˙
n
c
˙
n
)
=
(
0
λ
n
+
1
e
-
i
(
δ
-
Δ
)
t
e
-
S
/
2
0

λ
n
+
1
e
i
(
δ
-
Δ
)
t
e
-
S
/
2
0
T
e
e
i
ω
12
t
e
-
S

0
T
e
e
-
i
ω
12
t
e
-
S
0
)


×
(
a
n
+
1
b
n
c
n
)
.
The combination of the above coupled equations leads to a set of decoupled equations and their solutions could be obtained with the initial conditions a
n
+
1
(
0
)
=
F
n
+
1 and b
n
(
0
)
=
c
n
(
0
)
=
0.Analytically, the solutions can be directly given when phonon effect is not included forω
12
=
δ,  Δ
=
0,  δ
=
Δ, and ω
12
=
0; or the external optical field is in resonance with the zero-phonon line while the state |
1
〉 is in resonance with state |
2
〉 which indicates that the coherent population oscillations can persist, similar to the case without phonon effect, and expect that the expression in the Rabi like oscillating frequency and the interdot tunneling rate is renormalized by the exponents of -
S
/
2 and -
S [17]. We can see that electron-phonon coupling can make a significant contribution to the light-QDM interaction which can make the oscillation of the population of the state more drastic than that without the phonon effect [19].


## 3. Squeezing of the System

We introduce two orthogonal quadrature amplitude operatorsX
^
1
=
(
1
/
2
)
(
a
^
+
a
^
†
) and X
^
2
=
(
1
/
2
i
)
(
a
^
-
a
^
†
) satisfying the commutation relation [
X
^
1
,
X
^
2
]
=
i
/
2 which lead to
(5)
(
Δ
X
^
1
)
2
(
Δ
X
^
2
)
2
≥
1
16
according to Heisenberg’s uncertainty principle, with (
Δ
X
^
i
)
2
=
〈
X
^
i
2
〉
-
〈
X
^
i
〉
2
(
i
=
1,2
). The state of the field is said to be squeezed when one of the amplitudes X
^
i satisfies the relation Q
i
=
(
Δ
X
^
i
)
2
-
1
/
4
≤
0
(
i
=
1,2
). According to (3) we express the squeezing parameters for the two amplitudes as(6a)
Q
1
=
1
4
∑
n
‍
(
n
+
1
)
(
n
+
2
)
×
(
c
n
*
c
n
+
2
+
b
n
*
b
n
+
2
+
a
n
*
a
n
+
2
+
c
n
+
2
*
c
n
+
b
n
+
2
*
b
n
+
a
n
+
2
*
a
n
)
+
1
4
∑
n
‍
(
2
n
+
1
)
(
c
n
*
c
n
+
b
n
*
b
n
+
a
n
*
a
n
)
-
1
4
[
∑
n
‍
n
+
1
×
(
c
n
*
c
n
+
1
+
b
n
*
b
n
+
1
+
a
n
*
a
n
+
1
+
c
n
+
1
*
c
n
+
b
n
+
1
*
b
n
+
a
n
+
1
*
a
n
)
∑
n
‍
n
+
1
]
2
-
1
4
,
(6b)
Q
2
=
-
1
4
∑
n
‍
(
n
+
1
)
(
n
+
2
)
×
(
c
n
*
c
n
+
2
+
b
n
*
b
n
+
2
+
a
n
*
a
n
+
2
+
c
n
+
2
*
c
n
+
b
n
+
2
*
b
n
+
a
n
+
2
*
a
n
)
+
1
4
∑
n
‍
(
2
n
+
1
)
(
c
n
*
c
n
+
b
n
*
b
n
+
a
n
*
a
n
)
-
1
4
.Making the assumption that the optical field is initially in a monochromatic coherent state F
n
=
e
-
n
¯
/
2
n
¯
n
/
2
e
i
n
β
/
n
!, where the mean photon number of the coherent fields n
¯
=
|
α
|
2 and β is the phase, β
=
0 is chosen in the following.In order to investigate the squeezing in detail, we consider several factors that affect squeezing behaviors. First the temperature effect of the system is discussed, whereG
=
0.01 represents the electron-phonon interaction and Δ
=
δ
=
0.05
ω, ω
12
=
0, λ
=
0.2
ω, and T
e
=
0.2
ω; we choose different values of temperature T which directly modify the phonon population. In Figure 1 we show that, with the evolution of dimensionless time ω
t, the curves change significantly with the increase of temperature T. In the zero-temperature case (Figure 1(a)), the envelope of oscillation is sinusoidal but with a significant damping. In the time scale shown in the figure, there are more than three time regions where the system reaches squeezing for Q
1; however, the number of time ranges for the squeezing of Q
2 is even more but the amplitude of Q
2 is smaller than that of Q
1. We also notice that the oscillation frequencies of the squeezing parameters at higher temperatures are smaller than at lower ones. It is apparent that, for higher temperatures, T
=
50
ω
0 and T
=
100
ω
0, chances for the squeezing decrease for both Q
1 and Q
2. The physical explanation is obvious: the quantum properties are weakened for the increase of temperature; being a typical quantum phenomenon, squeezing is strongly suppressed by higher temperature.(Color online)Q
1,2 versus dimensionless time ω
t at different temperature when Δ
=
δ
=
0.05
ω, ω
12
=
0, G
=
0.01, T
e
=
0.2
ω, and λ
=
0.2
ω are considered.
(a)
(b)
(c)Now we set a fixed temperatureT
=
10
ω
0 (use this temperature hereafter) and assume the detuning δ
=
ω
12
=
0, electron-phonon interaction factor G
=
0.01, interdot tunneling T
e
=
0.2
ω, and field-QDM coupling λ
=
0.1
ω; then Figure 2 shows that when Δ varies from 0.01
ω to 0.05
ω the squeezing of the states significantly decreases, indicated by both Q
1 and Q
2 curves. The biggest squeezing appears for the smallest Δ; we find that the maximum squeezing reaches 24% (12%) for Q
1
(
Q
2
) when Δ
=
0.01
ω while the squeezing reduces to 2% (2.4%) when Δ increases to 0.05
ω. Also we find that, with the growth of Δ, the periodicity vanishes for long time scale (not shown in the figure) which means that the gradual enhancement phonon effect will lead to the irregular oscillations of the squeezing curves. The biggest squeezing happens around ω
t
=
40 (20) for Q
1 (Q
2) at small Δ and, after the time around ω
t
=
40, the system will not go back to the squeezed state any more.(Color online)Q
1,2 versus dimensionless time ω
t for different Δ when T
=
10
ω
0, δ
=
ω
12
=
0, G
=
0.01, T
e
=
0.2
ω, and λ
=
0.1
ω are chosen.
(a)
(b)
(c)It is interesting to speculate how the squeezing changes with detuningω
12 at fixed temperature and its time-dependent behaviors. In this case, we choose Δ
=
0 and ω
12 is ranging from 0.01
ω to 0.1
ω; T
e
=
0.2
ω, T
=
10
ω
0, and λ
=
0.1
ω are fixed as previously indicated. Noticing from Figure 3 clearly that squeezing decreases with the increase of ω
12, the biggest squeezing for Q
1
(
Q
2
) in ω
12
=
0.01
ω is 24% (12%) while it decreases to 12% (8%) when ω
12
=
0.03
ω, and notice, from Figure 3(d), however, there is almost no squeezing when ω
12
=
0.1
ω right after the system evolves. The curves in the figure also show that the squeezing of Q
1 is stronger than Q
2 regardless of ω
12 being small or big.(Color online)Q
1,2 varies with dimensionless time ω
t for different ω
12, when δ
=
Δ
=
0, T
=
10
ω
0, T
e
=
0.2
ω, and λ
=
0.1
ω are chosen.
(a)
(b)
(c)
(d)Previously we suppose that one or two parameters ofδ, ω
12, and Δ are zero and get some properties of the squeezing in different regimes. Now, to study the general case that both δ and ω
12 are nonzero and effect of Δ is included, we show the squeezing parameters in Figure 4 with three sets of values for ω
12 less than, equal to, and greater than δ separately. From the figure we find that when ω
12
<
δ, the squeezing of Q
2 is greater than Q
1 and the biggest squeezing for Q
1 (Q
2) is about 4
% (8
%); then with the continuous increasing of ratio ω
12
/
δ we find that squeezing for Q
2 is suppressed and eventually vanishes when ω
12
=
3
δ. Notice that there are two regions for X
1 being squeezed when ω
12
<
δ while the number of regions of squeezing reduces to one if the ratio of ω
12
/
δ increases; besides, the squeezing depth and duration of the first region nearly remain unchanged.(Color online)Q
1,2 versus dimensionless time ω
t for different detunings ω
12 and δ with the same parameters chosen as previously.
(a)
(b)
(c)Despite the cases that the mean photon numbern
¯
=
1 discussed above, it is significant to consider the effect of mean photon number n
¯ on the squeezing; we choose Δ
=
δ and states |
1
〉 and |
2
〉 are in resonance. When n
¯
=
1, we find that the oscillation for Q
1,2 is periodical with damping in the time range and the squeezing parameter evolves regularly; the biggest squeezing for Q
1 is around 25% happening at ω
t
=
38 while around 21% at ω
t
=
170 for Q
2. With the time evolution, the field can still be squeezed in the long time scale. When it comes to the bigger n
¯ cases, we find that, after the system reaches squeezing, the curves almost linearly increase monotonically, which correspond to the so-called Cummings collapse region [21, 22]. We find that the biggest squeezing will be higher than that in n
¯
=
1 case. If we want to obtain the biggest squeezing, the laser-QDM interaction time will be longer for larger n
¯.The discussion and results above are reliable and they can be implemented in labs. Now we consider the parameters that are used in InAs self-assembled QDM under coherent laser excitation and find that the squeezing for weak and strong tunneling is 6.4% and 22%, respectively, where we chooseω
=
1.6 eV, λ
=
1
×
1
0
-
3 eV, ω
12
=
0.1
×
1
0
-
3 eV, δ
=
0.1
×
1
0
-
3 eV, Δ
=
0, T
e
=
0.1
×
1
0
-
3 eV (weak tunnel), or 5
×
10
-
3 eV (strong tunnel) [23–28]; we find that the squeezing in weak tunneling is greater than that in strong tunneling case which shows that the coupling of the laser field and the QDM is equivalently weakened.


## 4. Conclusion

In this paper we have investigated the field squeezing of the quantum-dot molecule Jaynes-Cummings model. Using the appropriate approximation we give the Hamiltonian of the system describing the field-QDM interaction and solve the related equations afterwards. By analytical and numerical processes, we show influence of the various parameters of the system on the squeezing. We show that the squeezing generally decreases with time. It is shown that, because of the quantum nature being suppressed, the amount of squeezing becomes smaller as temperature rises, and the periodicity of the squeezing parameter curves is destroyed. The squeezing vanishes rapidly when the phonon effect is enhanced which shows that the phonon effect is distinct in this field-QDM interaction model. Despite these factors, increasing the ratio of detuningω
12 to δ can weaken the squeezing. In addition, the initial mean phonon numbers can play an important role in the squeezing; the big number makes the squeezing behavior obscure. Compared with the atomic assembled counterpart, the QDM has its advantage that is more convenient for the experimental manipulation and this field-QDM model opens up the new possibility of studying the light squeezing and allows its use in tunable semiconductor quantum-dot system.



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*Source: 395836-2014-07-03.xml*