Displacement and Squeeze Operators of a Three-Dimensional ... - arXiv

Displacement and Squeeze Operators of a Three-Dimensional Harmonic Oscillator and Their Associated Quantum States

Mehdi Miri, Sina Khorasani School of Electrical Engineering Sharif University of Technology P. O. Box 11365-9363 Tehran, Iran Fax: +9821-6602-3261 Email: [email protected]

Abstract We generalized the squeeze and displacement operators of the one-dimensional harmonic oscillator to the three-dimensional case and based on these operators we construct the corresponding coherent and squeezed states. We have also calculated the Wigner function for the three-dimensional harmonic oscillator and from the analysis of time evolution of this function, the quantum Liouville equation is also presented. Further properties of the quantum states including Mandel’s parameters are discussed as well.

Keywords: coherent states, phase space, squeezed states, operator algebra

1

and quadrature squeezing

1. Introduction The operator theory of harmonic oscillators [1] constitutes the groundwork of the elaborate quantum optical theory of photons. The quantization of electromagnetic radiation can be explained elegantly in terms of creator and annihilator operators, which operate on the corresponding energy levels [2-4]. Due to the second-order potential of harmonic oscillators, they can easily provide a direct bridge between classical optics and quantum optics through the phase-space Wigner functions [5], which are of extreme importance in the tomography of classical and non-classical lights [6-8]. Following the definition of coherent states put forward by Glauber [2-4], as the eigenstates of the annihilator operator, many studies have been done in order to generalize the concept of coherent states and the so-called squeezed states [5, 9]. Among these include an alternative definition of the generalized photon coherent states [10], which introduce a modification of the squeezing operator to describe higherorder interactions. In another report [11] the authors consider the generalization of coherent states and their superpositions connected through unitary transformations, where the transformation maps the ground state of the harmonic oscillator (vacuum state) onto an arbitrary superposition of

2 coherent states.

Since the successful demonstration of squeezed states of light in 1985 by Bell Laboratories [12], squeezed states have attracted much interest because of their possibility to significantly suppress the quantum noise, which is generally believed to be originated by the zero-point fluctuations of the vacuum [5]. Currently, squeezed states are routinely produced at laboratories using both solid-state and semiconductor lasers [13] and in high- cavities [14]. Similarly, generalizations or extensions to the concept of squeezed states have been considered in numerous researches. Nieto [15] was the first to discuss the explicit functional forms for the squeeze and time-displacement operators and their applications, as successive multiplications of exponentials of simple operators. Bialynicki-Birula [16,17] presented a discussion of squeezed states of a generalized infinitedimensional harmonic oscillator, when the ground state wave function takes on a Gaussian form. He furthermore presented the corresponding Wigner function and discussed its relativistic properties. As another generalization of the simple one-dimensional harmonic oscillator, the problem of damped harmonic oscillator because of its time-dependent Hamiltonian was proposed and considered by Um et. al. [18], and they presented closed form expressions for squeeze and displacement operators. Also, Sohn and Swanson [19] have recently obtained exact transition elements of the squeezed harmonic oscillator when

2

the generalized Hamiltonian describes two-photon processes, using Bogoliubov transformations. Fakhri [20] considered the three-dimensional (3D) harmonic oscillator and Morse potentials, and showed that the constructed Heisenberg Lie superalgebras would lead to multiple supercharges. In his analysis, he analyzed the 3D harmonic oscillator in the spherical system of coordinates. Finally, Fan and Jiang [21] have constructed three mutually commuting squeeze operators, which are applicable to three-mode states. In this paper, we revisit the 3D harmonic oscillator and obtain generalized expressions for the corresponding coherent and squeezed states, starting from the Cartesian coordinates in which the harmonic oscillator can be easily factorized. We also present closed-form simple expressions which explicitly represent the corresponding displacement and squeeze operators, and the corresponding generalized Mandel’s

parameter is obtained for the generalized squeezed state in the form of a vector.

We show that how proper definition of vector operators and variable could greatly simplify the notations of operators and eigenstates.

2. Coherent states and the displacement operator 2.1. Wigner function for 3D harmonic oscillator We can calculate wave function of three-dimensional (3D) harmonic oscillator directly from the Schrödinger equation, with the diagonalized potential given by

2.1

2

. Now let | , ,

Here, without loss of generality one may assume that

denote the

energy eigenstates of 3D harmonic oscillator, hence for the corresponding annihilation and creation operators we have | , ,

√ |

| , , | , ,

1, ,

2.2

a

√ | ,

1,

2.2

b

√| , ,

1

2.2

c

| , ,

√

1|

1, ,

2.2

d

| , ,

√

1| ,

1,

2.2

e

| , ,

√

1| , ,

2.2

f

3

1

Hence, the eigenfunctions will be

1

| , ,

Ψ

√2

!

1 2

exp

! !

H

H

H

2.3

⁄ . We can find the corresponding Wigner function for this system from the definition of

where

the Wigner function as

W|

Here,

1

,

, ,

exp

2

·

k represents the dummy integration variable. In the

is the density operator and | , ,

case of pure state with

W|

, ,

1

,

, , | gives

exp

2

2.4

·

Ψ

Ψ

2.5

The Wigner function of 3D harmonic oscillator will take the form

W|

, ,

1

, L

in which L

exp

2

L

2

L 2

2.6

is the Laguerre function of order ; see appendix A for the detailed derivation of (2.6). For

the generation of coherent states, we must apply a suitable displacement operator to the ground state of 3D harmonic oscillator. In doing so, we need to generalize the method of [15] in construction of 3D displacement operator. 2.2. Construction of coherent state The ground state of a 3D harmonic oscillator is given by

4

|

Ψ

in which the ground state |

1 2

exp

2.7

0,0,0 . Now we define the

is defined using the null integer triplet

displacement operator as exp

exp

exp , with

Here, the displacement vector

will be shown, the order of displacements along , , and

,

2.8 , and

being complex constants. As

is irrelevant. This is because of the obvious

relations ,

,

,

0, ,

,

, ,

2.9

0,

2.9

In trying to find a compact form for this operator we start from the Baker-Campbell-Hausdorff relation [5], which reads

exp

exp

exp

exp

1 2

,

2.10

given that

,

,

,

,

0

2.11

Hence the displacement operator is simplified into the compact form exp

·

·

2.12

where the vector creation and annihilation operators are defined by

5

2.13

a

2.13

b

to the ground state |

The application of the displacement operator | where |

|

results in

2.14

is defined as the generalized coherent state in 3D. Also, from the properties of

and

one can

further observe that 1 2

exp

The position representation of |

|

·

exp

exp

·

·

2.15

will be

1 2

exp

√2

√2 1 2

exp

√2

2.16

√2

The direct application of the displacement operator also can be simply shown to equally result in the triple infinite series of the generalized coherent state as

|

|

exp

exp

1 2

·

1 2

·

1 ! ! !

, ,

·

! ! !

, ,

·

| , ,

·

|

2.17

2.3. Over-completeness of coherent states As one of the important properties of coherent sates we can examine the over-completeness of the proposed coherent sates. A set of states are called over-complete if they form a complete set and are not orthogonal. We first consider the completeness of coherent states: ∞

∞

| ∞

∞

|

| ∞

|

exp ∞

6

1 2

·

exp

1 2

·

∞

, ,

| , !

, ,

Re

where

∞

Im

;

,

, , |

2.18

! ! ! ! !

, , . Using the change of variables:

exp

;

, ,

2.19

results in: ∞

, ,

∞

| , !

, ,

, , |

,

! ! ! ! !

∞

exp ∞

;

exp

It is known that

2

exp

2.20

2

, so using

;

, , , we get:

∞

|

|

∞ ∞

, ,

| ,

, !

,

, |

! !

∞

∞

exp

exp

∞

which can be easily simplified by using the identity ∞

exp

∞

∞

∞ exp ∞

! into the expression:

2.21

∞

| ∞

∞

|

| ,

,

,

, |

2.22

, ,

Therefore the proposed coherent sates constitute a complete set. Now we examine their non-orthogonality by considering the inner product of two different coherent states |

7

and |

:

|

exp

1 2

·

exp

exp exp exp

∞

,

· , ,

!

, ,

, | , ,

! ! ! ! !

∞

1 2

·

1 2

·

1 2

∞

1 2

·

!

, ,

·

·

·

! !

· 1 2

exp

·

2.23

Hence, we obtain the squared magnitude of the inner product as: | |

|

exp

·

0

2.24

which declares that 3D coherent states are not orthogonal, but their inner product tends to vanish, when |

| is sufficiently large. Equations (2.22) and (2.24), establish, therefore, that the proposed coherent

sates are over-complete.

2.4. Quantum Liouville equation in 3D Now we attempt to find the quantum Liouville equation for the generalized 3D harmonic oscillator system of interest. So we start from time evolution of our six-dimensional (6D) Wigner function. We have the Von Neumann equation for the time evolution of density operator as [1,5]

,

with

2.25

representing the Hamiltonian of the 3D harmonic oscillator. Starting from this equation we can

show that 1 2

1 2

1 2

,

1 2

With substitution of (2.19) in the definition of Wigner function we get

8

2.26

W , ,

Here,

and

2.27

respectively correspond to kinetic and potential energies in terms of Moyal functions and

introduce a Fourier transform as in [5]. The derivation closely follows the approach in [5], however, we employ the generalized 3D expressions for functions and operators. Hence,

and

will be given by the

expressions

1

1 2

exp

2 1 2

, ,

· 1 2

,

, , 2.28

a

and 1

exp

2 1 2

, ,

The potential energy operator

· 1 2

,

, , 2.28

b

is similarly defined as in [5]. Now we need to calculate

and

in terms

of the Wigner function and its higher-order derivatives. First we consider the kinetic energy term, which gives rise after some mathematical manipulations to the following equation for the kinetic energy term 1

·

W , ,

2.29

Now consider potential energy term. From the 3D Taylor expansion near , we have:

1 2

1 !

1 · 2

Therefore we obtain

9

2.30

1 2

1 2

2

2

·

!

2.31

and

1 2

1 2

2

2

·

1 !

2.32

We finally have the closed-form expression

2

1 2

·

1 !

W , ,

2.33

With substitution of (2.29) and (2.33) in (2.27) we get the Liouville's equation for the time-evolution of the Wigner function in 3D in the compact form

1

·

W , ,

2

1 2

1 !

·

W , ,

For the 3D harmonic oscillator in general case, the potential

2.34

is second-order in . So for the

harmonic oscillator, the right-hand-side of the Liouville's equation is equal to zero. Hence, the quantum Liouville's equation for 3D harmonic oscillator will be simply 1

·

·

W , ,

0

2.35

2.5. Time Evolution of Coherent State The Hamiltonian of 3D harmonic oscillator is time independent, so for the temporal evolution of the coherent state we can write down

|Ψ

| , ,

exp , ,

10

, , |Ψ

0

2.36

Defining the expansion coefficients as Ω

, , |Ψ

, ,

0

2.37

we get after some algebra

Ω

, ,

exp

1 2

·

2.38

√ ! ! !

On the other hand 3 | , , 2

| , ,

2.39

After simplifying we have

|Ψ

exp

3 2

√ ! ! !

, ,

exp

1 2

3 2

Ψ

| , ,

·

2.40

from which we obtain

|Ψ

exp

2.41

From this relation we see that the time evolution of coherent state is also a coherent state, and also after one period

of oscillation, the state vector phase change is

3 .

2.6. Position representation of coherent state In the below we try to find a compact form for position representation of coherent state of 3D harmonic oscillator. This results in

11

|Ψ exp

1 3 2

1 2

exp

·

·

exp √2

·

2.42

Using the definitions √2

Re Im

√2 3 2

Φ

· 2

1

·

2

1 2

·

2.43

a

2.43

b

2.43

c

Re

·

2.43

d

Finally, the complete form of position space representation of coherent state is Ψ

,

|Ψ exp

2

·

exp

for real

Here, as for the case in 1D problem

·

exp

Φ

2.44

will take on real values, otherwise it will be complex.

3. Squeezed states and the squeeze operator Now we try to find functional form of squeeze operator and squeezed state of 3D harmonic oscillator and position representation of this squeezed state. For 1D case, the squeeze operator is defined as

exp

1 2

1 2

where in general is a complex number

12

3.1

| |

3.2

Expanded form of 1D squeezing operator is therefore

exp

1 2

tanh| |

sech| | !

sech | |

1

1 2

exp

tanh| |

3.3

If we use notation of [15] as 1 √2 ̂

1 √2

3.4

a

3.4

b

the new form of squeezing operator will take the form

exp

1 2

3.5

2

In the expanded form we have

exp

sinh| | 2| |

exp

ln

exp

sinh| |

3.6

2| |

where

cosh| |

s sinh| | | |

| |

cos

2

| |

sin

2

3.7

In generalization of this concept to 3D case we consider 3D squeezing as independently squeezing of wave function of harmonic oscillator in the three

,

, and

dimensions. So for the 3D harmonic

oscillator this method can be applied directly resulting as 3.8

13

,

Here,

operate only on , , and

, and

dimensions, respectively, and hence the

order of their appearance is irrelevant as will be shown shortly. We have 1 2 1 exp 2 1 exp 2

1 2 1 2 1 2

1 2

1 2

exp

3.9

a

3.9

b

3.9

c

Therefore

exp

1 2

1 2

exp

1 2

1 2

exp

3.10

Now let the following definitions hold

̂

1 √2 ̂

1 √2

3.11

a

3.11

b

, , . We furthermore we can show that

in which

,

,

,

,

0

3.12

where ,

, ,

,

,

With subsequent use of (3.12) we can show that

,

,

14

0

3.13

a

,

,

,

, ,

,

,

,

0

,

,

0

,

,

,

0

3.13

b

3.13

c

3.13

d

, ,

From equation (3.13) and after using (3.12), and the Baker-Campbell-Hausdorff relation one can easily show that the squeeze operator in 3D takes the more compact form

exp

1 2

3.14

With the help of the definitions of vectors 3.15

a

3.15

b

3.15

c

we can find a rather compact form for squeezing operator as

exp

1 2

3.16

The following commutation relations clearly hold

,̂ ̂

̂, ̂

,

̂ , ̂

, ,

, ,

from which the alternate form of the squeeze operator is obtained

15

̂ , ̂

0

3.17

exp

1 2

·

·

3.18

In the last equation we have used the short-hand notations Re

3.19

a

Im

3.19

b

̂ ̂

3.19

c

3.19

d

3.19

e

4. Construction of squeezed states For the generation of squeezed state we must apply the squeeze operator and then coherent operator on the ground state of harmonic oscillator. Here in this process, we use the notation of [15] employed in (3.6). This results in |

| , |

Notice that

3.20

represents the squeezed vacuum. Following the previous definitions and after some

algebra we reach at the position representation of the squeezed state as Ψ

| , 1

exp

2

exp

·

1

exp

1

exp

Here,

·

2 1

exp

2 ,

2

, and

1

2

, where

3.22

16

a

3.21

sinh 2 exp

3.22

b

, ,

and

are elements of the vectors

and

⁄√2, and

defined in (3.19),

3.23 cosh

sinh

exp

cos

2

tan

a sin

exp 3.23

2

3.23

b

c

, , For the detailed derivation of the (3.21), please refer to the Appendix B. 4.1. Further properties of squeezed states In this section we will consider two important properties of squeezed states; quadrature squeezing parameter and Mandel’s

parameter. For 1D squeezed states these two are defined as scalars, while for

the proposed 3D states we define the generalized quadrature squeezing and Mandel’s vector form. In the following we start with Mandel’s Mandel’s

parameters in the

parameter.

“as a measure of departure of the variance of the photon number n from the variance of a

Poisson process” was first proposed and calculated by Mandel [22, 23]. Δ

For an arbitrary state,

;

Δ

3.24

can be negative, zero, or positive, which respectively infers a super-Poissonian,

Poissonian or sub-Poissonian statistics [24]. It should be added here that Mandel has shown that, one should expect the squeezed states to show sub-Poissonian photon statistics through normal detection schemes [23].

17

For our 3D squeezed states, we define a vectorial Mandel’s Mandel’s

,

parameter,

,

where

is the

parameter related to squeezing in the direction. Note that the proposed squeezed state here

can also be represented as the multiplication of three squeezed sates: Ψ

1

Ψ

, ,

Ψ

exp

Ψ

3.25

1

exp

exp

2

y Ψ

Ψ

;

2

, ,

3.26

Now by using the results of [24] for 1D squeezed state, we can show that: | |

cos | |

and

sin sinh

2 sinh

cosh

1;

, ,

3.27

are defined in (3.23) and | |

1 2

3.28

tan

3.28 3.28

2 , , In this case, Mandel’s

parameter for squeezing in each direction (

;

, , ) can be negative, zero

or positive which means the statistics of squeezed states in that particular direction is super-Poissonian, Poissonian or sub-Poissonian respectively. Surface plots of the Mandel’s Figure 1, as a function of dependence on the angle cosh

sinh

and , while retaining when

parameter are illustrated in

as a constant. As it can be seen, there is no

0. For this special case, one can easily check from (3.27) that

.

Similarly, we can also define vectorial quadrature operator: 1 2

18

3.29

a

1 2 where

and

3.29

b

are defined in (2.13). In 1D squeezed state variances of quadrature operators are measures 1/2

of squeezing. In fact for a 1D squeezed state with quadrature

and

1/2

operators squeezing exists if [25]: 1 4

Δ

1 4

Δ

3.30

Again for our 3D squeezed state, we can calculate variances of elements of vectorial quadrature operators from the results of [24] for 1D squeezed state:

Δ

Δ

, Δ

, Δ

3.31

Δ

Δ

, Δ

, Δ

3.31

Δ Δ

1 4 1 4

cos sin

sin

2

cos

2

3.31

2

3.31

2

, , , , , , squeezing exists if:

Thus for 3D squeezed state, in direction

Δ

1 4

Δ

1 4

;

Plots of squeeze parameters (3.31c) and (3.31d) versus

, ,

and

3.32

are shown in Figs. 2 and 3, respectively as

surface and contour diagrams. As it can be seen, squeezed states happen over the domains in which (3.32) 1 4

holds, and any of the squeeze parameters fall under . Evidently, the transformation subplots for Δ

and Δ

switches the

, due to the algebraic forms of the expressions (3.31c) and (3.31d).

19

Furthermore, Figure 4 shows the domain of squeezed Δ

versus de-squeezed Δ

,

states,

,

respectively, filled in with color contours, and left blank. The borders could be explicitly found by solving (3.31c) and (3.31d) for Δ

. This gives after simplifications to the fairly compact expression

,

tan

;

2

, ,

3.32

which defines the borders separating the squeezed and de-squeezed states.

5. Conclusions In this paper, we presented new closed-form expressions for coherent states and squeeze operators of a generalized harmonic oscillator potential in three spatial dimensions. We defined proper creation and annihilation operators and succeeded in presenting simple expressions for the corresponding displacement and squeeze operators.

Appendix A: Derivation of Wigner function of 3D harmonic oscillator The position representation of | , ,

| , ,

Ψ

state 3D harmonic oscillator reads:

1 √2

!

1 2

exp

! !

H

H

H

A. 1

Placing the above in the definition of Wigner function in (2.5) gives:

W|

, ,

1

,

2 ·

1

H

exp

! !

1 2

exp 1 2

!

2

1 2

exp 1 2 1

1 2

H ·

·

20

1 2

H H .2

1 2

H H

1 2

1 2

exp

! 1 2

1 2

exp 1 2

H

1

1 2

exp 1 2

H

exp √ 2

exp

1 2

1 2

H

1 2

exp

1 2

1 2

H

1 2

1 2

exp

1 2

1 2

H

.5

we have:

1 4

exp

!

1 2

. By changing

Consider for example the first integral

1 2

.4

exp

!

1 2 .3

exp

!

2

1 2

H

1 2

exp

1 2

1 2

.6

and now by using the algebraic manipulation: 1 4

1 2

2

and change of variables

2

.7

2 :

exp

1 2

!

√ exp

H

.8

H

from symmetry of Hermite polynomials we know that H

21

1 H

. So

exp

1

1 2

!

√ H

exp

H

.9

Also it is known that:

1 2

1 !√

exp

H

H

L

2

. 10

where L is the Laguerre polynomial of order n. Therefore

1 exp

L

2

. 11

Repeating the same procedure for Iy and Iz results in:

W|

, ,

1

, L

exp

2

L

2

L 2

. 12

Appendix B: Derivation of Position representation of 3D squeezed state From (2.8) and by using the notation of [15] we can write the 3D displacement operator in this new form:

exp

2

exp

̂ exp

22

;

, ,

.1

where ̂ and

are defined in (3.11) and

and

are define above the (3.23). Furthermore as it is shown

in (3.10) 3D squeeze operator can also be shown to be:

exp

1 2 ̂

̂

;

, ,

.2

Our proposed squeezed state is constructed from ground state of a 3D harmonic oscillator (vacuum state) as in (3.20). So its position representation can be calculated from: |

| ,

Ψ 1

exp

1 2

.3

From the previously used commutation relation it is obvious that:

Ψ

1

exp

1 2

1 2

exp

exp

1 2

B. 4

Using [15] gives: 1 2

1

exp

2

1

exp

exp

2

.5

, , which directly results in the position representation of the squeezed state as:

Ψ

1

exp

2 exp

·

exp

1

exp

·

2

1

exp

2

23

1 2

B. 6

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25

Figure Captions Figure 1. Mandel’s

parameter plotted versus

Figure 2. Squeeze parameters versus

and for various values of .

and .

Figure 3. Contours of Squeeze parameters versus

and .

Figure 4. The domain of squeezed states (filled with contours) as separated from de-squeezed states (white).

26

α =1

Mandel Parameter Q

Mandel Parameter Q

α =0

25 20 15 10 5 2

20 10 0 2

3

0 r

-2

3

0

2

2

1 0

r

δ

-2

30 20 10 0 2 3

0 -2

30 20 10 0 2 3 2

1 0

δ

0

2 r

0

α =3

Mandel Parameter Q

Mandel Parameter Q

α =2

1

r

δ

Figure 1

27

-2

1 0

δ

Squeeze Parameter < Δ I2 2>

Squeeze Parameter < Δ I1 2> 12 10 8 6 4 2

2 0 2 3

r

r -2

-2

0

0

Figure 2

28

1

φ

12 10 8 6 4 2

2 0 2 3

1

φ

Contours of 2 5 2.5

r

1

1

0.5 0.25

0 0.05

0.1

0.15 0.2

-1

-2

0

0.5

1

1.5

2

2.5

3

φ Contours of 2 5 2.5 1

1

r

0.5 0.25

0

0.2

0.15

-1

-2

0

0.5

1

1.5

φ

Figure 3

29

2

2.5

0.1

0.05

3

Borders of Squeezed States 2 1.5 1

r

0.5 0 -0.5 -1 -1.5 -2

0

0.5

1

1.5

φ

Figure 4

30

2

2.5

3