Strong Mechanical Squeezing and its Detection

# Strong Mechanical Squeezing and its Detection

## Abstract

We report an efficient mechanism to generate a squeezed state of a mechanical mirror in an optomechanical system. We use especially tuned parametric amplifier (PA) inside the cavity and the parametric photon phonon processes to transfer quantum squeezing from photons to phonons with almost 100% efficiency. We get 50% squeezing of the mechanical mirror which is limited by the PA. We present analytical results for the mechanical squeezing thus enabling one to understand the dependence of squeezing on system parameters like gain of PA, cooperativity, temperature. As in cooling experiments the detrimental effects of mirror’s Brownian and zero point noises are strongly suppressed by the pumping power. By judicious choice of the phases, the cavity output is squeezed only if the mirror is squeezed thus providing us a direct measure of the mirror’s squeezing. Further considerable larger squeezing of the mirror can be obtained by adding the known feedback techniques.

###### pacs:
42.50.Wk, 42.50.Lc, 03.65.Ta, 05.40.-a

## I Introduction

Cavity optomechanics is based on the radiation pressure interaction between light and mechanical resonators at macroscopic scales Aspelmeyer14 (). Currently, with the rapid progress of practical technologies in cavity optomechanics, the mechanical resonator can be cooled down close to the quantum ground state Cleland (); Teufel (); Chan (). Thus it is possible to explore quantum effects in macroscopic systems, including superposition state Bose (); Simon (), entanglement Kim (); Plenio (); Agarwal09 (), squeezing of light Fabre (); Mancini (); Regal (); FlorianNPJ (); Agarwal14 (); Qu (); Kilda (), squeezing of the mechanical resonator Agarwal91 (); Dodonov (); Braginsky (); Mari (); Li (); Liao (); Kronwald (); Zoller (); Sumei (); Ruskov (); Florian (); Bowen (); Vitali14 (); Nori (); Vanner (); Benito (); Wollman (); PRL (); PRX (); Bowen1 (); Pontin (); Vinante (), etc.

The quantum squeezing of mechanical modes is important as it can be used to improve the precision of quantum measurements Cave (). There have been many theoretical proposals for generating squeezing of the mechanical mode Agarwal91 (); Dodonov (); Braginsky (); Mari (); Li (); Liao (); Kronwald (); Zoller (); Sumei (); Vitali14 (); Nori (); Vanner (); Benito (); Ruskov (); Florian (). Several experiments have reported squeezing of the mirror to different degrees. Since mechanical motion is represented by an oscillator, the most direct way to produce squeezing is via the well known methods used to squeeze the oscillator motion. One of the early proposals was to modulate the frequency of the oscillator Agarwal91 (); Dodonov (); Braginsky (). While this is the simplest, it is not easy to adopt for many different kinds of mechanical systems currently in use. Alternate methods to overcome this limitation have been suggested. These include modulation of the external laser Mari (); Li (); Liao (); use of a two tone drive one red detuned and the other blue detuned Kronwald (). One can use a broad band squeezed optical field and couple it into an optomechanical cavity to transfer optical squeezing into mechanical squeezing Zoller (); Sumei (). This method works very well and more than 50% squeezing of the mirror can be obtained Zoller (); Sumei (). This requires efficient coupling and a highly squeezed broad band field and thus has its own limitations. A more direct way is to have a parametric amplifier placed inside the optomechanical cavity so that the squeezing of the cavity field is generated inside the cavity. These squeezed cavity photons can interact directly with the red-detuned pump laser to produce squeezing of the mechanical mode. This is the main theme of the present work. The degree of the mechanical squeezing will be limited by the squeezing produced by the PA. However one can use the previously used methods like the single quadrature feedback scheme Vinante () or the weak measurement Bowen (); Pontin () to substantially increase the mirror’s squeezing.

While we concentrate on optomechanical couplings linear in mirrorâs displacement, the squeezing of the mirror in quadratically coupled OMS has been investigated. In this case one can use a bang-bang technique to kick the mirror mode Vitali14 (); Vanner (); use the Duffing nonlinearity Nori (); use two tone driving Benito ().

In this paper, we propose a scheme to generate the momentum squeezing of the movable mirror by placing a degenerate PA inside a Fabry-Perot cavity with one moving mirror. The PA is pumped at twice the frequency of the anti-Stokes sideband of the driving laser interacting the movable mirror. It is shown that the squeezing of the cavity field induced by the PA can be transferred to the movable mirror. The achieved momentum squeezing of the mirror depends on the parametric gain, the parametric phase, the power of the input laser, and the temperature of the environment.

The paper is organized as follows. In Sec. II, we describe the model, give the quantum Langevin equations, and the steady-state mean values. In Sec. III, we linearize the quantum Langevin equations, derive the stability conditions, calculate the square fluctuations in position and momentum of the movable mirror. In Sec. IV, we discuss how the momentum squeezing of the movable mirror can be realized by using the PA inside the cavity. In Sec. V, we derive the analytical expression of the mean square fluctuation in the momentum of the movable mirror. In Sec. VI, we show how the mechanical squeezing can be measured by the output field. Our conclusions are given in Sec. VII.

## Ii Model

We consider a degenerate PA contained in a Fabry-Perot cavity with one fixed mirror and one movable mirror, as shown in Fig. 1. A degenerate parametric amplifier (PA) is generally used to produce a squeezed light Walls (); Kimble (). We have shown earlier that a PA inside an optomechanical system can improve the cooling of the movable mirror Sumei1 (). It can also make the observation of the normal-mode splitting Girvin (); Aspelmeyer () of the movable mirror and the output field more accessible Sumei2 (). The fixed mirror is partially transmitting, while the movable mirror is totally reflecting.

The separation between the two mirrors is . A cavity field with resonance frequency is driven by an external laser with frequency and amplitude . The intracavity photons exert a radiation pressure force on the movable mirror, causing the optomechanical interaction between the cavity field and the movable mirror. Meanwhile, the movable mirror is in contact with a thermal bath in equilibrium at temperature , which induces a thermal Langevin force acting on the movable mirror. Under the action of these two forces, the mirror makes small oscillations around its equilibrium position. The movable mirror is treated as a quantum-mechanical harmonic oscillator with effective mass , frequency , and energy decay rate . In the degenerate PA, we assume that a pump field at frequency interacts with a second-order nonlinear optical crystal, thus the signal and the idler have the same frequency . We assume that the gain of the PA is , depending on the power of the pump driving the PA, the phase of the pump driving the PA is . The Hamiltonian of the system in the rotating frame at the laser frequency is given by

 H = ℏ(ωc−ωl)c†c−ℏg0c†c(b+b†)+ℏωm(b†b+12) (1) +iℏεl(c†−c)+iℏG(eiθc†2e−2iωmt −e−iθc2e2iωmt),

where and are the annihilation and creation operators of the cavity mode, satisfying the commutator relation , and are the annihilation and creation operators of the mechanical mode, satisfying . The optomechanical interaction strength is in unit of Hz, where is the zero point motion of the movable mirror. The is related to the power of the laser by with being the cavity decay rate due to the leakage of photons through the partially transmitting mirror. In Eq. (1), the first and third terms describe the energies of the optical mode and the mechanical mode, respectively, the second term describes the linear optomechanical coupling between the cavity field and the movable mirror, depending on the photon number in the cavity, the fourth term gives the driving of the input laser, the last term represents the coupling between the cavity field and the PA. The physical process can be illustrated in Fig. 2. Fig. 2(a) shows the frequency relation among the pump photon at frequency , the cavity photon at frequency , the squeezed photon at frequency from the PA, and the phonon at frequency . Fig. 2(b) shows that a phonon at frequency is spontaneously created by a red-detuned pump photon at frequency interacting with an input noise photon at frequency . Fig. 2(c) shows that a cavity photon at frequency is produced when a red-detuned pump photon at frequency interacting with a phonon at frequency . Fig. 2(d) shows that a squeezed phonon at frequency is generated when a red-detuned pump photon at frequency interacts with a squeezed photon at frequency from the PA.

According to Heisenberg motion equation and considering the quantum and thermal noises, we obtain the quantum Langevin equations

 ˙b = ig0c†c−iωmb−γm2b+√γmbin, ˙c = −i(ωc−ωl)c+ig0c(b+b†)+εl+2Geiθc†e−2iωmt (2) −κc+√2κcin.

Here is the boson annihilation operator of the thermal noise with zero mean value, its nonzero correlation functions are

 ⟨b†in(t)bin(t′)⟩=nthmδ(t−t′), ⟨bin(t)b†in(t′)⟩=(nthm+1)δ(t−t′), (3)

where is the initial mean thermal excitation number in the movable mirror, is the Boltzmann constant. Moreover, is the input quantum noise operator with zero mean value, its nonzero correlation function is

 ⟨c†in(t)cin(t′)⟩=nthcδ(t−t′), ⟨cin(t)c†in(t′)⟩=(nthc+1)δ(t−t′), (4)

where is the initial mean thermal excitation number in the optical mode. The steady state mean values of the system operators are

 cs = εlκ+iΔ, bs = ig0|cs|2γm2+iωm, (5)

where is the effective cavity detuning from the frequency of the input laser in the presence of the radiation pressure, depending on the mechanical motion. The is the steady-state amplitude of the cavity field, determines the steady-state displacement of the movable mirror. The mean numbers of the cavity photons and the mechanical phonons are given by and , respectively.

## Iii Radiation pressure and quantum fluctuations

In order to show the movable mirror in a squeezed state, we need to calculate the position and momentum fluctuations of the movable mirror. Here we are interested in the strong-driving regime so that the intracavity photon number satisfies . Let and , where and are the small fluctuation operators around the steady state mean values, thus Eq. (2) can be linearized by neglecting higher than first order terms in the fluctuations Pina (). Introducing the slow varying fluctuation operators by , , , , we obtain the linearized quantum Langevin equations

 δ˙~b = i[g∗δ~ce−i(Δ−ωm)t+gδ~c†ei(Δ+ωm)t]−γm2δ~b +√γm~bin, δ˙~c = −κδ~c+ig[δ~be−i(ωm−Δ)t+δ~b†ei(ωm+Δ)t] (6) +2Geiθδ~c†e2i(Δ−ωm)t+√2κ~cin,

where is the effective optomechanical coupling rate, depending on the power of the input laser. We assume that the driving field is red-detuned from the cavity resonance (), thus the anti-Stokes scattered light is nearly resonant with the cavity field. And we assume that the system is working in the resolved sideband limit , the mechanical quality factor is high , the mechanical frequency is much larger than and . Under these conditions, the rotating wave approximation can be made, the fast oscillating term in Eq. (III) can be ignored, Eq. (III) can be simplified to

 δ˙~b = ig∗δ~c−γm2δ~b+√γm~bin, δ˙~c = −κδ~c+igδ~b+2Geiθδ~c†+√2κ~cin. (7)

Introducing the position and momentum fluctuations of the mechanical oscillator as and , and the amplitude and phase fluctuations of the cavity field as and , the amplitude and phase fluctuations of the input quantum noise as and , and the position and momentum fluctuations of the thermal noise as and , the equation (III) can be written as the matrix form

 ˙f(t)=Mf(t)+n(t), (8)

where is the column vector of the fluctuations, and is the column vector of the noise sources. Their transposes are

 f(t)T = (δQ,δP,δx,δy), n(t)T = (√γmQin,√γmPin,√2κxin,√2κyin); (9)

and the matrix is given by

 M=⎛⎜ ⎜ ⎜ ⎜ ⎜ ⎜⎝−γm20i2(g∗−g)−12(g+g∗)0−γm212(g+g∗)i2(g∗−g)i2(g−g∗)−12(g+g∗)−(κ−2Gcosθ)2Gsinθ12(g+g∗)i2(g−g∗)2Gsinθ−(κ+2Gcosθ)⎞⎟ ⎟ ⎟ ⎟ ⎟ ⎟⎠. (10)

The stability conditions of the system can be obtained by requiring that all the eigenvalues of the matrix have negative real parts. Applying the Routh-Hurwitz criterion stable1 (); stable2 (), we find the stability conditions

 14γ3m+2κ(κ2−4G2)+(2κ+γm)(|g|2+2κγm)>0, 2κγm(κ2−4G2)2+[(2κ+γm)2|g|2+(4κ+γm)κγ2m] ×(κ2−4G2)+γ3m4[κγ2m2+(2κ+γm)|g|2] +κγm(2κ+γm)[κγ2m+(2κ+32γm)|g|2]>0, 14γ2m(κ2−4G2)+|g|2(|g|2+κγm)>0. (11)

Note that the stability conditions are independent of the parametric phase . The system stays in the stable regime only if .

By taking the Fourier transform of Eq. (8) and solving it in the frequency domain, we obtain the expressions for the position and momentum fluctuations of the movable mirror

 δQ(ω) = A1(ω)xin(ω)+B1(ω)yin(ω)+E1(ω)Qin(ω) +F1(ω)Pin(ω), δP(ω) = A2(ω)xin(ω)+B2(ω)yin(ω)+E2(ω)Qin(ω) (12) +F2(ω)Pin(ω),

where

 A1(ω) = √2κid(ω){v(ω)[Gα−iu(ω)Im(g)]−i|g|2Im(g)}, B1(ω) = √2κd(ω){v(ω)[Gβ−u(ω)Re(g)]−|g|2Re(g)}, E1(ω) = √γmd(ω){[u(ω)2−4G2]v(ω)+|g|2u(ω)+GΓ}, F1(ω) = √γmd(ω)iG(g2e−iθ−g∗2eiθ), A2(ω) = √2κd(ω){v(ω)[Gβ+u(ω)Re(g)]+|g|2Re(g)}, B2(ω) = −√2κid(ω){v(ω)[Gα+iu(ω)Im(g)]+i|g|2Im(g)}, E2(ω) = √γmd(ω)iG(g2e−iθ−g∗2eiθ), F2(ω) = √γmd(ω){[u(ω)2−4G2]v(ω)+|g|2u(ω)−GΓ},

with , , , , , and

 d(ω)=[u(ω)v(ω)+|g|2]2−4G2v(ω)2. (14)

In Eq. (III), the first two terms in and are from the radiation pressure contribution, the last two terms are from the thermal noise contribution. In the absence of the optomechanical coupling , the movable mirror makes quantum Brownian motion because of the coupling to the environment, , . The spectra of fluctuations in the position and momentum of the movable mirror are defined by

 SZ(ω) = 14π∫+∞−∞dΩ e−i(ω+Ω)t[⟨δZ(ω)δZ(Ω)⟩ (15) +⟨δZ(Ω)δZ(ω)⟩],Z=Q,P.

By the aid of the nonzero correlation functions of the noise sources in the frequency domain,

 ⟨Qin(ω)Qin(Ω)⟩ = ⟨Pin(ω)Pin(Ω)⟩ = (nthm+12)2πδ(ω+Ω), ⟨Qin(ω)Pin(Ω)⟩ = −⟨Pin(ω)Qin(Ω)⟩=i22πδ(ω+Ω), ⟨xin(ω)xin(Ω)⟩ = ⟨yin(ω)yin(Ω)⟩ = (nthc+12)2πδ(ω+Ω), ⟨xin(ω)yin(Ω)⟩ = −⟨yin(ω)xin(Ω)⟩=i22πδ(ω+Ω),

we obtain the spectra of fluctuations in the position and momentum of the movable mirror

 SQ(ω) = [A1(ω)A1(−ω)+B1(ω)B1(−ω)](nthc+12) +[E1(ω)E1(−ω)+F1(ω)F1(−ω)](nthm+12), SP(ω) = [A2(ω)A2(−ω)+B2(ω)B2(−ω)](nthc+12) +[E2(ω)E2(−ω)+F2(ω)F2(−ω)](nthm+12),

where the first term proportional to in and is from the radiation pressure contribution, while the second term proportional to is from the thermal noise contribution. In the absence of the cavity field, the spectra of fluctuations in position and momentum of the movable mirror are given by , whose peaks are located at frequency zero with full width at half maximum. The mean square fluctuations and in the position and momentum of the movable mirror are determined by

 ⟨δZ(t)2⟩ = 12π∫+∞−∞dω SZ(ω),Z=Q,P. (18)

Without the optomechanical coupling, we find . For K, the movable mirror is in the ground state , . According to the Heisenberg uncertainty principle, the product of the mean square fluctuations and satisfies the following inequality

 ⟨δQ(t)2⟩⟨δP(t)2⟩≥|12[Q,P]|2, (19)

where . If either or is below , the state of the movable mirror exhibits quadrature squeezing. The degree of the squeezing can be expressed in the dB unit, which can be calculated by with being the momentum variance of the vacuum state and .

## Iv The mechanical squeezing

In this section, we numerically evaluate the mean square fluctuations in the position and momentum of the movable mirror given by Eq. (18) to show quadrature squeezing of the movable mirror under the action of the PA. The values of the parameters are chosen to be similar to those in the experiment demonstrating mechanical squeezing with two pumps Wollman (): , , the mechanical quality factor . For convenience, we define the optomechanical cooperativity parameter , which is proportional to the power of the external laser. From the numerical results, it is found that can not be less than , but can be less than . Therefore we focus on discussing here.

The mean square fluctuation as a function of the parametric gain for different parametric phases when and K is shown in Fig. 3. When , , the system is in the weak-coupling regime, and the conditions for the rotating wave approximation are satisfied. From Fig. 3, it is seen that =0.5 in the absence of the PA (), thus there is no squeezing in the momentum fluctuation of the movable mirror. In the presence of the PA (), can be less than 0.5 except . Hence the addition of the PA in the optomechanical system can realize the momentum squeezing of the movable mirror. Furthermore, it is observed that the minimum value of is the smallest when , which is at , the corresponding amount of the maximum momentum squeezing is about 49.4%, the degree of the squeezing is about dB. The squeezing of the cavity field in the absence of the optomechanical coupling is given in the Appendix. The maximum phase squeezing of the cavity field is about dB when and . Note that the maximum momentum squeezing of the movable mirror is equal to the maximum phase squeezing of the cavity field, but they happen at different parametric phases . The phase difference is related to the phase of and . Thus the squeezing of the cavity field is totally transferred into the movable mirror. This is because driving the system by the red-detuned laser in the resoved sideband limit makes the optomechanical interaction between the movable mirror and the cavity field like a beamsplitter interaction.

The mean square fluctuation as a function of the cooperativity parameter for different parametric phases when and K is shown in Fig. 4. In the absence of the optomechanical coupling () between the cavity field and the movable mirror, it is seen that . In the presence of the optomechanical coupling (), drops to about 0.320, 0.261, 0.417 for , respectively, thus the optomechanical coupling can lead to the momentum squeezing of the movable mirror. The corresponding degrees of the squeezing are about 1.94 dB, 2.82 dB, 0.79 dB for , respectively. It is noted that the momentum squeezing of the movable mirror almost keeps constant when the cooperativity parameter is larger than a certain value and it persists over a very wide range.

In this paragraph, we discuss previous results on mechanical squeezing. The mechanical squeezing is not larger than 3 dB in Mari (); Li (); Liao () as in this work. In the current work it is limited by the squeezing that a parametric device can produce. A relatively large mechanical squeezing can be achieved by feeding in squeezed light Zoller (); Sumei (). Here one gets about 6 dB squeezing by feeding in light with about 9 dB squeezing. The two tone driving as discussed in detail in Ref. Kronwald () can also produce large squeezing (more than 3 dB). For this, the intensity of the blue-detuned drive has to be close but smaller than the intensity of the red-detuned drive and the cooperativity parameter has to be large. The latter requirement should not be in conflict with the dropping of the nonresonant terms in the case of two tone driving. In addition, the mechanical squeezing beyond 3 dB can be created by quantum measurement and feedback to remove the effect of the quantum back action Ruskov (); Florian (). Several experiments have reported good mechanical squeezing. The best experimental mechanical squeezing is roughly 1.0 dB in Wollman (); PRL (); PRX (), 6.2 dB in Bowen1 (), 7.4 dB in Pontin (), and 11.5 dB in Vinante (), respectively. It is clear that additional methods are to be used to go beyond 3 dB squeezing. This is briefly discussed at the end of Sec. V.

We find that the amount of squeezing of the mechanical mirror is not very sensitive to the parameters. We next choose parameters corresponding to an optical cavity. We take , . The mean square fluctuation as a function of the parametric gain for different parametric phases when and K is shown in Fig. 5. When , , the system is in the weak-coupling regime, and the conditions for the rotating wave approximation are satisfied. It is seen that takes the smallest value 0.253 when and , which is similar to that in Fig. 3.

The mean square fluctuation as a function of the cooperativity parameter for different parametric phases when and K is similar to Fig. 4. In the presence of the optomechanical coupling, drops to about 0.320, 0.261, 0.416 for , respectively.

We next examine the effect of the Brownian noise on squeezing i.e. the effect of the temperature of the environment. We need the values of the cavity frequency and the mechanical frequency . We assume GHz and MHz Wollman (). The mean square fluctuation as a function of the parametric gain for different temperatures of the environment when and is plotted in Fig. 6. For 0 K, 10 mK, 20 mK, the corresponding initial mean thermal excitation numbers in the optical mode are 0, , and , respectively, the corresponding initial mean thermal excitation numbers in the mechanical mode are 0, 57.4, and 115.3, respectively. It is noted that increasing the temperature of the environment would decrease the momentum squeezing of the movable mirror. For example, when , K, 10 mK, , 0.395, respectively, the corresponding degrees of the squeezing are about 2.96 dB, 1.02 dB, respectively. When the temperature of the environment is increased to mK, is always larger than 0.5, thus the squeezing of the mechanical mode does not occur. We have confirmed that for the optical cavity case the results of Fig. 6 hold with almost no change. For brevity we do not present the figure for the optical cavity case.

The PA inside the OM cavity can produce a number of novel effects besides squeezing of the mirror and cooling. Some of these are generation of the genuine tripartite entangled states Xuereb (), enhancement of the precision of optomechanical position detection Peano (), enhancement of the effective optomechanical interaction strength Lu (); Nation (). The latter could become important for getting closer to single photon coupling regime.

## V Analytical Approach to Understand Mechanical Squeezing

In this section, we will present an analytical approach to understand the result of Sec. IV. In the weakly optomechanical coupling regime , in which the photons leak out of the cavity much faster than the optomechanical interaction, the cavity field follows the mechanical motion adiabatically. The adiabatical approximation can be made, thus . We obtain

 δ~c = 1κ2−4G2(iκgδ~b−i2Geiθg∗δ~b†+2Geiθ√2κ~c†in (20) +κ√2κ~cin).

Substituting into Eq. (III), we have

 δ˙~b = −(κ|g|2κ2−4G2+γm2)δ~b+2Geiθg∗2κ2−4G2δ~b† (21) +ig∗√2κκ2−4G2(2Geiθ~c†in+κ~cin)+√γm~bin.

In the absence of the PA or the cavity field , it is noted that does not depend on , thus the squeezing of the movable mirror does not appear. In the presence of the PA and the cavity field, depends on . This parametric coupling can lead to the squeezing of the movable mirror. Therefore, the PA in the cavity can realize the squeezing of the movable mirror.

In the parameter domain we are working the term in the coefficient of can be ignored. Let and we choose a value of such that ), then we write (21) as

 δ˙~b = −|g|2(1−G20)κδ~b−G0|g|2(1−G20)κδ~b† (22) +ig∗√2κ(1−G20)κ(G0eiθ~c†in+~cin)+√γm~bin.

From Eq. (22), we get the equation for the momentum fluctuation as

 δ˙P=−|g|2κ(1+G0)δP+h(t)+f(t), (23)

where the quantum Langevin forces are given by

 h(t) = √γm√2i(~bin−~b†in), (24) f(t) = g∗√κκ(1+G0)(~cin−~c†ineiθ). (25)

Using Eq. (25) and Eq. (II), we obtain the correlation function of

 ⟨f(t)f(t′)⟩=|g|2κ(1+G0)2(1+2nthc)δ(t−t′). (26)

The correlation function of can be calculated using (24) and (II).

 ⟨h(t)h(t′)⟩=γm2(1+2nthm)δ(t−t′). (27)

We now obtain the equation for using (23), (26), and (27) as

 ∂⟨δP2⟩∂t = −2|g|2κ(1+G0)⟨δP2⟩+|g|2κ(1+G0)2(1+2nthc) (28) +γm2(1+2nthm),

and therefore we get the analytical result for the squeezing of the quadrature in the steady state as

 ⟨δP2⟩=12(1+G0)(1+2nthc)+γmκ(1+G0)4|g|2(1+2nthm). (29)

For , , we find

 ⟨δP2⟩≈14(1+2nthc)+1800(1+2nthm), (30)

which gives values about 0.25, 0.40, and 0.55 for (), 10 mK (, ), and 20 mK (, ), respectively. These analytical results are in excellent agreement with the numerical results in Fig. 6 for close to but less than 0.5. A very important feature of the result (29) which is to noticed is the suppression of the Brownian noise by the cooperativity parameter . As we have mentioned earlier and as has been realized by several others Ruskov (); Florian (), the 3 dB limit can be broken by using the feedback mechanism as in Ref. Vinante (). Let be the dimensionless feedback gain parameter, then detailed calculations show that the squeezing given by Eq. (29) is reduced by a factor of . The maximum value of is limited by the stability of the dynamical equations. Thus an order to get 75% squeezing (6 dB), we need the condition . Still larger squeezing is achievable by increasing the feedback. Note that stability requires that should be not larger than .

## Vi The Detection of the Mechanical Squeezing

In this section, we analyze that the mechanical squeezing can be measured by the output field. The fluctuation of the cavity field can be obtained from Eq. (8). Using the input-output relation Walls (), we can get the fluctuation of the output field. Then we define the quadrature fluctuation of the output field as

 δzout(ω) = 1√2[δcout(ω)e−iϕ+δcout(−ω)†eiϕ