Dissipation-driven two-mode mechanical squeezed states in optomechanical systems

Dissipation-driven two-mode mechanical squeezed states in optomechanical systems

Abstract

In this paper, we propose two quantum optomechanical arrangements that permit the dissipation-enabled generation of steady two-mode mechanical squeezed states. In the first setup, the mechanical oscillators are placed in a two-mode optical resonator while in the second setup the mechanical oscillators are located in two coupled single-mode cavities. We show analytically that for an appropriate choice of the pump parameters, the two mechanical oscillators can be driven by cavity dissipation into a stationary two-mode squeezed vacuum, provided that mechanical damping is negligible. The effect of thermal fluctuations is also investigated in detail and show that ground state pre-cooling of the oscillators in not necessary for the two-mode squeezing. These proposals can be realized in a number of optomechanical systems with current state-of-the-art experimental techniques.

I Introduction

Quantum squeezing and entanglement have been observed in a number of atomic and photonic systems and are expected to play an increasing role in applications ranging from measurements of feeble forces and fields to quantum information science (1); (2); (3); (4). For example, it has been know for over three decades that squeezed vibrational states are of importance for the measurement beyond the standard quantum limit of the weak signals expected to be produced e.g. in gravitational wave antennas (5).

Although achieving such effects in macroscopic systems remains a major challenge due in particular to the increasing rate of environment-induced decoherence (6), recent progress toward the ground-state cooling of micromechanical systems (7); (8); (9); (10); (11) may change the situation significantly in the near future. In particular, the characterization of quantum ground-state mechanical motion (12), the quantum control of a mechanical resonator deep in the quantum regime and coupled to a quantum qubit (13), and the demonstration of optomechanical ponderomotive squeezing (14) are important steps toward the broad exploration of quantum effects in truly macroscopic systems (15); (16); (17); (18); (19); (20); (21); (22); (23). Several proposals have been put forward to generate mechanical squeezing in an optomechanical oscillator, including the injection of nonclassical light (24), conditional quantum measurements (25), and parametric amplification (26); (27); (28); (29). In all cases, decoherence and losses are a dominant limiting factor in the amount of squeezing that can be achieved.

A new paradigm in quantum state preparation and control has recently received increased attention. Its key aspect is that it exploits quantum dissipation in the generation of specific quantum states. Quantum reservoir engineering has been proposed to prepare desirable quantum states (30); (31); (32); (33) and perform quantum operations (34), and the creation of steady-state entanglement between two atomic ensembles by quantum reservoir engineering has been experimentally demonstrated (35). This dissipative approach to quantum state preparation presents the double advantage of being independent of specific initial states and of leading to steady states robust to decoherence.

Here, we propose to exploit cavity dissipation to generate the steady-state two-mode squeezing of two spatially separated mechanical oscillators. These states are also entangled states of continuous variables, a basic resource in quantum information precessing. We propose specifically two different setups. In the first one two mechanical oscillators are placed inside a two-mode optical resonator, while in the second one the mechanical oscillators are located in two separate single-mode cavities coupled by photon tunneling. The cavities are driven in both cases by amplitude-modulated lasers. In the first model we show analytically that for appropriate mechanical oscillator positions and pump laser parameters the mechanical oscillators can be driven into a stationary two-mode squeezed vacuum by cavity dissipation, provided that mechanical damping is negligible. In the second case a two-step driving sequence can likewise give rise to a steady two-mode mechanical squeezed vacuum state. The effect of thermal fluctuations on the resulting squeezed states is also investigated in detail.

The remainder of this paper is organized as follows. Section II introduces our first model of two mechanical oscillators coupled by radiation pressure to the field of a common two-mode optical resonator. It then discusses how to prepare a two-mode mechanical squeezed state. Section III shows that cavity damping can likewise be exploited to create a squeezed mechanical state of two mechanical oscillators in separated single-mode cavities. Finally, Section IV is a conclusion and outlook.

Ii Mechanical oscillators in a single two-mode cavity

ii.1 Model and equations

We first consider an extension of the “membrane-in-the-middle” arrangement of cavity optomechanics (36) where two mechanical oscillators, modeled as vibrating dielectric membranes of identical frequencies , are located inside a driven two-mode optical resonator, as illustrated in Fig. 1. The mechanical modes are characterized by the bosonic annihilation operators and the cavity modes, at frequencies , by annihilation operators . These modes are driven by amplitude-modulated lasers of frequencies . The Hamiltonian of the driven cavity-oscillators system reads ()

(1)

where are the time-dependent amplitudes of the pump lasers. Their specific forms will be given later. The single-photon optomechanical coupling constants (36), where is the length of the cavity, are the identical masses of the membranes, and . Here and are the reflection coefficients and equilibrium positions of the two membranes and the wave numbers of the cavity modes.

For an appropriate combination of cavity length and membrane positions of the membranes, see Fig.1, it is possible to find a situation such that the “symmetrical” and “antisymmetric” optomechanical coupling strengths satisfy the equalities

(2)

as discussed in Ref. (37). Introducing then the new bosonic annihilation operators

(3a)
(3b)

the Hamiltonian becomes , where

(4)

In terms of the normal operators , the system is therefore decoupled and reduces to two independent single-membrane optomechanical systems.

Figure 1: Schematic plot of two vibrating membranes () placed at appropriately-chosen positions in a driven cavity with two frequency-nondegenerate resonant modes ().

Further decomposing the operators and as

(5)

and with and one can linearize the Hamiltonians to get

(6)

where

with , and the effective optomechanical coupling strengths are given by

(7)

The density matrix of the sub-system composed of the cavity mode and the normal mode satisfies the master equation

(8)

where is the cavity dissipation rate and the mechanical damping rate, taken to be the same for both oscillators. The mean thermal phonon number is , with the Boltzmann constant and the temperature.

ii.2 Stationary two-mode mechanical squeezed vacuum via cavity dissipation

We now show how cavity dissipation can be exploited to prepare the stationary two-mode mechanical squeezed vacuum of the vibrating membranes. To this end we consider an effective optomechanical coupling strength of the form

(9)

where and are constants. This situation can be realized by a pump laser of the form discussed in Section II.3.

For weak optomechanical coupling we have , so that if the cavity-laser detuning and the modulation frequency are

(10)

the transformation and reduces the Hamiltonian to

(11)

This form can be further simplified for a mechanical frequency , in which case the rapid oscillating terms can be neglected and

(12)

This Hamiltonian describes the coupling of the cavity field to the normal mode simultaneously via parametric amplification – through the term proportional to – and via a beam splitter-type coupling – through the constant contribution . It is known that the first term in the Hamiltonian (12) leads to photon-phonon entanglement and phononic heating of the normal mode , while the second term results in quantum state transfer between the cavity mode and the mechanical mode as well as to mechanical cooling (cold damping). To ensure the stability of the system, the coupling strengths must satisfy the inequality , that is, cooling should dominate over anti-damping.

When absorbing a laser photon the parametric amplification term results in the simultaneous emission of a photon into the cavity mode and a phonon in the normal mode , while the beam-splitter interaction corresponds to the annihilation of a photon and the emission of a phonon. We now show that the combined effect of these processes is the generation of steady-state single-mode squeezing of the normal mechanical mode , or equivalently of two-mode squeezing of the original modes and .

We proceed by first performing the unitary transformation

(13)

where the squeezing operator

(14)

with

(15)
(16)

For the master equation (8) becomes then

(17)

where

(18)

with

(19)

describes quantum-state transfer between the cavity mode and the mechanical mode in the transformed picture. It can be inferred from that master equation that in the transformed picture and for the cavity mode and the mechanical mode asymptotically decay to the ground state

(20)

Simply reversing the unitary transformation (13) we have then that in the steady-state regime the normal mode is indeed in the squeezed vacuum state

(21)

It is possible to adjust the amplitude and phase of the optomechanical coupling coefficient  (9) in such a way that the squeezing parameters satisfy the conditions

(22a)
(22b)

in which case the two normal modes and exhibit the same amount of steady-state squeezing, but in perpendicular directions. With Eqs. (3) and (21) we then have

(23)

where we have introduced the two-mode squeezing operator

(24)

and . This two-mode squeezed vacuum of the mechanical oscillators can be thought of as the output from a 50:50 beam splitter characterized by the unitary transformation (3), the two inputs being the normal modes squeezed in perpendicular directions. This shows that for the dissipation of the intracavity field can be exploited to prepare pure two-mode mechanical squeezed vacuum state. The minimum time required for preparing such states can be evaluated from the eigenvalues of Eq (17),

For symmetric parameters , , and one finds for .

ii.3 The choice of pump lasers

Next we consider the choice of pump laser amplitudes that result in the time-dependent optomechanical coupling (9), and the specific form (22) that results in the pure two-mode mechanical squeezing (23). From Eq. (7) an obvious starting ansatz is

(25)

where are the initial phases of two components with amplitudes and are modulation frequencies. The corresponding amplitudes and of the cavity and mechanical modes are

(26)

It is difficult to find exact solutions of these equations in general. For the case of the weak optomechanical coupling strengths , however, approximate analytical solutions can be found by expanding the amplitudes and in powers of as and . Substituting these into Eqs. (26) and for the time , , , and one then finds (higher-order corrections can be derived straightforwardly)

(27a)
(27b)
(27c)
(27d)

with the phases

(28)

For coupling strengths , for example for , , and , we find and . We can therefore set , and the effective optomechanical coupling strength takes the required form (9) for

(29)

Finally, Eqs. (28) and (22b) give

(30)

ii.4 Thermal fluctuations

For finite mechanical damping, , the mechanical modes and are no longer be in a pure squeezed state, but rather in a two-mode squeezed thermal state. In the state, we find from Eqs.  (3) and (8)

(31a)
(31b)

where , , and

(32)

The quantum correlations between the mechanical oscillators can be quantified by the sum of variances (3); (38)

(33)

where are quadrature operators with local phase . A value of is a signature of Einstein-Podolsky-Rosen (EPR)-type correlations between the two mechanical modes, with corresponding to the ideal quantum mechanical limit (3). In our case we find that is minimum for the choice of local phases . In the long-time limit it is equal to

(34)

We first observe that for we have and hence , showing that in the absence of cavity dissipation the oscillators are just prepared in the thermal state imposed by their mechanical coupling to the environment. This confirms that cavity dissipation is an essential component of this realization of steady-state two-mode mechanical squeezing. From Eq. (34), steady-state squeezing requires that

(35)

In practice, it is important to be able to operate at as high a number of mean thermal phonons as possible. This can be achieved by decreasing while keeping the “cooperative parameter” . From Eq. (32) and for the realistic case , reduces approximately to

(36)

indicating that by increasing the coupling frequency while keeping the ratio fixed it is possible to increase the value of which is approximately given by

(37)

As a concrete example, for a cavity dissipation rate of , a mechanical damping , and coupling strengths and , we have . This indicates that two-mode mechanical squeezing is robust against thermal fluctuations and ground-state precooling of the mechanical modes may not be necessary.

Iii Mechanical oscillators in separate single-mode cavities

Figure 2: (a) Two vibrating membranes () in separate single-mode cavities () are optically coupled by either an optical fiber. (b) Two evanescent-wave-coupled optomechanical crystal nanocavities.

In this section we show that the same dissipative approach can also be utilized to generate a two-mode squeezed state of two mechanical oscillators in separate single-mode cavities. The specific example that we consider consists of two identical single-mode cavities of frequency , optically coupled to via fiber (a) or evanescent-wave coupling (b), see Fig. 4. Each cavity field is driven by a modulated laser and optomechanically coupled to a mechanical oscillator of frequency . Adopting the same symbols as before the Hamiltonian of that system reads

(38)

where account for the optomechanical coupling strengths, assumed to be identical, and describes the coupling between the two cavities. Here we consider two pump fields of equal frequency and time-dependent amplitude

(39)

For that symmetrical situation, both cavity fields have the same amplitude and the linearized Hamiltonian is

(40)

where

(41)

and the detuning for the weak optomechanical coupling. By introducing the new bosonic operators

(42a)
(42b)

the Hamiltonian separates as before into the sum of two uncoupled Hamiltonians, , where

with effective detunings and . The dynamics of the two independent optomechanical sub-systems are governed by the same master equations as before, see Eq. (8).

In contrast to the preceding case, though, in the two-cavity setup it is not possible to simultaneously achieve the single-mode squeezing of the normal modes and since there is only one driving laser field and one set of control parameters (). However, for sufficiently weak mechanical decoherence it is possible in principle to implement a two-step process that can still achieve that goal.

For the first step we choose the frequencies and such that

(44)

and the phases

(45)

where is arbitrary. With the transformation and , the Hamiltonians reduce to

(46a)
(46b)

For , the non-resonant terms in these Hamiltonians can be neglected and they reduce to and , respectively. For the mode this is formally the same situation as encountered in Section IIB. Neglecting as before the mechanical damping, , cavity dissipation brings likewise that normal mode into a steady-state single-mode squeezed vacuum for long enough time, and at the same time mode simply decays into the vacuum, i.e.,

(47a)
(47b)

where , as defined before, is a time long enough that steady state has been reached. After the first step the mechanical oscillators and are therefore prepared in a pure two-mode squeezed state, although not a standard two-mode squeezed vacuum. That latter goal can be achieved in a second step by changing the frequency and phase of the pump laser at time so that

(48)

and the phases

(49)

For the weak optomechanical coupling, we then have that , which means that the mode evolves freely in the state of Eq. (47a), while . After a time both the normal modes and are therefore in steady-state single-mode squeezed vacua,

(50a)
(50b)

and the mechanical modes and are in the two-mode squeezed vacuum state,