Abstract
Precision measurement of nonlinear observables is an important goal in all facets of quantum optics. This allows measurementbased nonclassical state preparation, which has been applied to great success in various physical systems, and provides a route for quantum information processing with otherwise linear interactions. In cavity optomechanics much progress has been made using linear interactions and measurement, but observation of nonlinear mechanical degreesoffreedom remains outstanding. Here we report the observation of displacementsquared thermal motion of a micromechanical resonator by exploiting the intrinsic nonlinearity of the radiationpressure interaction. Using this measurement we generate bimodal mechanical states of motion with separations and feature sizes well below 100 pm. Future improvements to this approach will allow the preparation of quantum superposition states, which can be used to experimentally explore collapse models of the wavefunction and the potential for mechanicalresonatorbased quantum information and metrology applications.
Introduction
A key tool in quantum optics is the use of measurement to conditionally prepare quantum states. This technique, often simply referred to as ‘conditioning’, has been applied to generate nonGaussian quantum states for confined microwave fields^{1}, travelling optical fields^{2,3} and superconducting systems^{4}. In addition, quantum measurements are of vital importance to many quantum computation protocols^{5}. In cavity optomechanics, light circulating inside an optical resonator is used to manipulate and measure the motion of a mechanical element via the radiationpressure interaction^{6}. After an optomechanical interaction performing a measurement on the light can then be used to conditionally prepare mechanical states of motion. This form of state preparation can be understood as a combination of Bayesian inference, that is, updating our knowledge of the system, and backaction (see Supplementary Note 1 for an introduction). Subsequent measurements following the conditioning step can be used to characterize the state prepared. Such mechanical conditioning has been performed with measurements of the mechanical position^{7,8,9}, however, thus far, conditioning has not been performed with a measurement of a nonlinear mechanical degree of freedom. One exciting prospect is to dispersively couple the optical field to the mechanical position squared^{10}, which could enable the detection of phonon number jumps^{10,11} and thus demonstrate mechanical energy quantization. Here we implement an alternative approach that instead utilises the optical nonlinearity of the radiationpressure coupling, as was proposed in ref. 12. Such a positionsquared measurement can ultimately be used to prepare a mechanical superposition state^{13} as the measurement does not reveal the sign of the mechanical position. Studying the dynamics of superposition states can be used to test models of decoherence beyond standard quantum mechanics^{12,14,15,16,17,18,19} and for the development of mechanical quantum sensors.
For the optomechanical system of interest in this work, the intracavity Hamiltonian in a frame rotating at the optical carrier frequency is H/ħ=ω_{M}b^{†}b+g_{0}a^{†}a(b+b^{†}) where a(b) is the optical (mechanical) annihilation operator, ω_{M} is the mechanical angular frequency and g_{0} is the zeropoint optomechanical coupling rate. Quite generally, optomechanics experiments todate have focused on dynamics describable by a linearized model of the radiationpressure interaction^{6}, where the photon number operator is approximated by and N is the mean intracavity photon number. In this approximation, mechanical displacements give rise to displacements of the optical phase quadrature leaving the optical amplitude quadrature unchanged. Fundamentally, however, the radiationpressure interaction is nonlinear^{12,20}, and generates mechanical positiondependent rotations of the intracavity optical field. For small changes in the mechanical position, the optical phase quadrature changes linearly in proportion to the mechanical displacement, and the optical amplitude quadrature reduces in proportion to the mechanical displacement squared. By choosing which optical quadrature to observe with homodyne detection, one may selectively measure the mechanical displacement or displacementsquared^{12}. Since a displacementsquared measurement does not distinguish between positive and negative displacement, mechanical superposition states may be prepared by measurement^{13}. A necessary requirement for the optical interaction to effect a direct measurement of the displacementsquared is that the mechanical motion is negligible during the intracavity photon lifetime, that is, operation in the badcavity regime (, where κ is the optical amplitude decay rate of the cavity). This should be contrasted to other approaches operating in the resolved sideband regime , where cavityaveraged displacementsquared interactions have been predicted to allow the observation of the mechanical phononnumber^{10,11}. In this work we observe optomechanical dynamics arising from the nonlinearity of the radiationpressure interaction and, utilizing this nonlinearity, perform nonGaussian state generation by measurement of displacementsquared mechanical motion.
In the badcavity regime, the intracavity field can be approximated as , where quantifies the optomechanical interaction strength, ξ is the intracavity noise term and is the mechanical displacement in units of the mechanical quantum noise (Supplementary Note 2). Taylor expanding the intracavity field, the timedependent optical output quadratures are then
where , and . Conventionally, experimental optomechanics have focused on the leading, linear term in the expansion of the phase quadrature. In this linearized picture, only a single spectral peak at the mechanical resonance frequency is expected. Higherorder terms in mechanical displacement, however, give rise to spectral peaks at the respective multiples of the mechanical resonance frequency which are only described by the full nonlinear optomechanical Hamiltonian. Precision measurement of these higherorder terms enables the conditional preparation of nonGaussian states which, in a quantum regime, produces highly nonclassical states^{21}.
Here we use the intrinsic nonlinearity of the radiationpressure interaction to effect a displacementsquared measurement of the motion of a mechanical oscillator. We use this measurement to conditionally prepare classical bimodal states of mechanical motion from an initial roomtemperature thermal state. Further we theoretically show that this continuous measurement approach, with the introduction of feedback, may be extended to a quantum regime, allowing preparation of macroscopic quantum superposition states of mechanical motion.
Results
Optomechanical system
A schematic of our nonlinear optomechanics experiment is shown in Fig. 1. We use a nearfield cavity optomechanical setup^{22}, where a mechanical SiN nanostring oscillator^{23} is placed in close proximity to a 60μm diameter optical microsphere resonator and interacts with the optical cavity field via the optical evanescent field (Fig. 1c). The nanostring has dimensions 1,000 × 10 × 0.054 μm (length × width × thickness) and a fundamental mechanical resonance frequency of ω_{M}/2π=100.2 kHz. From the known dimensions and density we estimate an effective mass of m=0.86 ng. A continuouswave fibre laser, operating at 1,559 nm, is locked on resonance with a whisperinggallery mode of the microsphere. We measure an optical amplitude decay rate of κ/2π=25.6 MHz and a mechanical linewidth of γ/2π=0.7 Hz. An evanescent optomechanical coupling of 7.6 MHz/nm was determined (Methods section), corresponding to a coupling rate of g_{0}/2π=75 Hz. We use ∼2 μW of optical drive power resulting in an intracavity photon number N=2.4 × 10^{4}. A fibrebased Mach–Zehnder interferometer is used to perform homodyne detection and thereby selectively measure a quadrature of the optical output field.
Figure 2a,b show the observed homodyne noise power spectra for both optical phase and amplitude quadratures at the mechanical frequency and the second harmonic, respectively. At ω_{M} (Fig. 2a) we observe a Lorentzian peak in the phase quadrature from the thermal motion of the oscillator, which corresponds to a rootmeansquare (RMS) displacement of 124 pm corresponding to a thermal occupation of . The thermal noise is resolved with 85 dB of signal relative to the homodyne noise power when the signal is blocked, which corresponds to an ideal displacement sensitivity of 1.3 × 10^{−15} m Hz^{−1/2}. In practice, the signal beam is not shot noise limited due to cavity, acoustic and laser noise which raise the measurement imprecision by roughly an order of magnitude. By setting the interferometer phase to measure the optical amplitude quadrature, the linear measurement of mechanical motion is suppressed by ∼45 dB. At this quadrature, information about the displacementsquared mechanical motion is observed in a frequency band centred at 2ω_{M} (Fig. 2b). We observe a Lorentzian peak with a linewidth of 1.5 Hz, which to within the measurement uncertainty, is equal to twice the linewidth at ω_{M} (Supplementary Note 3 and Supplementary Fig. 1). The signaltonoise at this frequency is 65 dB relative to the homodyne noise, which corresponds to a calibrated ideal displacementsquared sensitivity of 3.3 × 10^{−24} m^{2} Hz^{−1/2}.
Figure 2c shows the band power in the first and second harmonics as a function of the interferometer phase. The powers in each band are expected to follow sine and cosine squared functions (fitted). The observed suppression of the linear measurement allows an upper bound to be placed on the phase instability of the cavity and interferometer locks of at most 5 × 10^{−3} rad. Figure 2d shows the observed relative noise powers up to the fourth harmonic of the mechanical frequency. The expected noise powers can be computed with the Isserlis–Wick theorem (Supplementary Notes 3 and 11), which show excellent agreement with experiment.
State preparation and readout
Of primary interest in this work is the lowest order nonlinear measurement term in the optical amplitude quadrature, proportional to . To describe this quantitatively we introduce the slowly varying quadratures of motion, X and Y, defined via X_{M}(t)=X(t) cosω_{M}t+Y(t) sin ω_{M}t. The mechanical displacementsquared signal can then be written as:
where for later convenience, the displacementsquared quadratures of motion are defined and . By inspection, it can be seen that the quadratic measurement has spectral components both at DC and 2ω_{M}. Higherorder terms in the expansion equations (1 and 2) can in principle contribute to the signal at 2ω_{M}, however since , the quadratic term is the only term to contribute substantial power at 2ω_{M}. Consequently, linear and quadratic components of the measurement can be spectrally separated and therefore, at an appropriate homodyne angle, measured simultaneously.
To perform both state preparation and state reconstruction we set a homodyne angle of π/4, which allows simultaneous highfidelity linear measurement (for state reconstruction) and quadratic measurements (for state preparation). The photocurrent generated at the homodyne output is digitized into 4 second blocks at a sample rate of 5 × 10^{6} s^{−1}, which are then filtered numerically at ω_{M} and 2ω_{M} to obtain the respective quadratures of motion in each frequency band as detailed in Supplementary Note 4. For a large signaltonoise ratio, the squares of each quadrature of motion can be estimated from the measurements of P and Q via the nonlinear transformations and , where the tildes denote the (noise inclusive) measurement outcomes of the respective quantity. These transformations allow the recovery of a classical estimate of without knowledge of the signal at DC. Figure 3a plots the estimates thus obtained from the 2ω_{M} signal against the cosine mechanical position quadrature, , obtained from the measurement at ω_{M}. A clear quadratic relationship between the two measurements is observed, validating the displacementsquared nature of the 2ω_{M} peak.
Conditioning based on the outcome of the quadratic measurement can be used to prepare nonGaussian states. In the most basic approach, conditioning and , for some constant C, will produce a bimodal state with a separation of . However, to make more efficient use of the available data, we additionally perform a mechanical phase rotation for each sample in the measurement record. First, at each discrete sample we find a rotation by a phase angle 2φ such that the new rotated variable is equal to zero. As a result, in the frame rotated by the half angle, φ, correlation between the two mechanical quadratures and is conditionally eliminated. Second, we condition on a particular magnitude of (Methods section). This operation localizes the phasespace distribution of the reconstructed state to two small regions as shown in Fig. 3b, with a separation dependent on the conditioning value. These states, although classical, are evidently bimodal and nonGaussian. Further details of this protocol are contained in Supplementary Note 5 and Supplementary Fig. 2. Extending this protocol to a regime where the quadratic measurement rate dominates all decoherence processes, a macroscopic quantum superposition state can be generated. Indeed, as detailed later, a simulated state prepared in this way is shown in Fig. 4b.
Comparison of effective coupling rates
At present, in opto and electromechanics, techniques towards measurement of nonlinear observables of mechanical motion include coupling to twolevel systems^{24} and radiationpressure interactions coupling to the displacementsquared, such as the ‘membraneinthemiddle’ (MiM) approach^{10}. In the latter approach, a mechanically vibrating element is appropriately placed within an optical standing wave in a cavity to give a displacementsquared dispersive coupling of the form H_{int}/ħ=μ_{0}a^{†}a(b+b^{†})^{2}, where μ_{0} is the zeropoint quadratic coupling rate. This interaction, when operating in the resolved sideband regime, in principle allows for the observation of quantum jumps in the mechanical phonon number. Experiments exhibiting this type of coupling include dielectric membrane systems^{10,25,26}, trapped cold atoms^{27}, trapped microspheres^{28} or doubledisk structures^{29}. However it should be noted that in these systems, quadratic coupling rates μ_{0} are typically orders of magnitude smaller than attainable linear coupling rates g_{0}.
In contrast to a displacementsquared Hamiltonian coupling, the scheme employed here gives an effective quadratic coupling rate of (ref. 12), which should be compared with μ_{0} defined above. For the modest linear coupling achieved in the present work, we have a /2πκ=2.2 × 10^{−4} Hz. Crucially, since the coupling rate in our scheme scales as , substantial gains are possible by improving g_{0}. For instance, the coupling rate for a stateoftheart evanescently coupled nanostringmicrocavity system as described in ref. 30 is Hz and for a stateoftheart electromechanical system^{31} is Hz. Furthermore, other optical systems with exceptional linear coupling rates^{32} should have quadratic coupling rates using our scheme as high as 160 Hz. In comparison, a stateoftheart MiM system as described in ref. 26 has a quadratic coupling rate of μ_{0}/2π=6.0 × 10^{−3} Hz. Thus a significantly larger effective quadratic coupling is possible using our protocol. Noteably, the quadratic measurement rate resulting from this fundamental coupling may be boosted by a coherent optical drive, which makes entering the quantum regime more feasible.
Requirements for nonclassical behaviour
In all measurementbased quantum state preparation schemes, the measurement rate must dominate the sum of all decoherence process rates due to coupling of the system to the environment. In MiM displacementsquared coupling protocols, even in a zerotemperature environment, this introduces the challenging requirement of singlephoton strong coupling (g_{0}/κ>1)^{11}. By contrast, our scheme offers a route to relax this stringent criterion. In our scheme, when state conditioning is performed with only the quadratic motion component of the detected signal, decoherence from the linearized radiationpressure noise on the mechanics precludes nonclassical state generation outside of a singlephoton strong coupling regime, similar to MiM (Supplementary Note 6). However, by including feedback, this form of decoherence can, in the limit of perfect detection efficiency, be completely eliminated (Supplementary Note 7). This is because the amplitude quadrature measurement records not only the X^{2} mechanical motion, but also the optical intracavity amplitude fluctuations near the mechanical resonance frequency. Since these fluctuations drive the linearized radiation pressure backaction on the mechanics, suitable feedback to the motion of the mechanical oscillator can cancel this radiationpressure noise. Additionally, with this feedback, the mechanical dynamics reduce to a similar form as with the displacementsquared dispersive Hamiltonian coupling. In the realistic case of imperfect detection efficiency η, the decoherence can be suppressed up to a factor of 1−η. This results in the coupling strength requirement to reach a quantum regime (see Supplementary Notes 7,9,10 and Supplementary Figs 3–5 which quantify the effect of decoherence arising from linear interactions). For example, with a detection efficiency of η=0.98 the singlephoton coupling rate need only be one tenth of the strong coupling requirement. Additionally, the quadratic measurement rate must dominate rethermalisation, that is, . Provided the coupling strength criterion is satisfied, rethermalisation can be made insignificant with only modest intracavity photon numbers in cryogenic systems.
Based on these criteria, the quantum regime of our scheme can be achieved with current atomoptomechanical systems. For instance, quantum superposition states of motion could immediately be implemented with the approach in ref. 33, provided the detection efficiency exceeds 10%. Furthermore, solidstate optomechanical devices have seen rapid gains in performance over the past decade, with both optical and microwave systems now operating within three orders of magnitude of the singlephoton strong coupling regime. For example, an effective coupling rate of g_{0}/κ=0.04 has recently been achieved in a superconducting microwave optomechanical device^{34}, and with modest modifications, it is expected the system will approach the strong coupling regime. When g_{0}/κ=0.04, the generation of quantum superposition states using our protocol requires detection efficiency on the order of 99.7%. However, with a one order of magnitude improvement in the coupling rate, the required detection efficiency drops to 76%, such that in combination with state of the art amplifiers^{35}, nonclassical state generation using our protocol could be realised. A full list of parameters is provided in Supplementary Table 1.
Technical limitations may also play a role in the implementation of our protocol in a quantum regime. For example, fluctuations or offsets in the interferometer phase or cavity lock will result in linear coupling to the environment, and therefore an additional source of decoherence. Linear coupling can also be introduced undesirably due to the presence of other mechanical modes in the system, which mix via the optical nonlinearity with the mode of interest. Indeed the sum beat between the two mechanical modes in Fig. 2a is observed as the +4.3 kHz peak in Fig. 2b. These additional linear decoherence channels are expected to be negligible compared with the decoherence due to linear radiation pressure backaction as detailed Supplementary Note 8. The currently unutilised DC component of the homodyne signal constitutes an additional technical decoherence channel. However, unlike the decoherence mechanisms discussed above, this channel is nonlinear, carrying information about phonon number rather than mechanical position. This can be seen from the expansion of the quadratic motion in terms of the creation and annihilation operators, , and identifying the number operator n=b^{†}b plus a constant as the DC part. As a result, loss of the DC information generates phase diffusion on the mechanical state. Somewhat strikingly, the nonclassicality of states generated by X^{2} measurement can in fact be quite robust against this form of decoherence. In Supplementary Note 9, the effect of phononnumber decoherence of an initial superposition state is analysed, showing that Wigner function negativity is preserved even in the presence of a complete loss of phonon number information to the environment. This result is illustrated in Fig. 4c,d and in further detail in Supplementary Fig. 6.
Quantum trajectory simulation
Finally, to elucidate the precise effect of the combination of all identified decoherence processes on the state conditioned via continuous quadratic measurement, a master equation simulation of our system was performed. The results for a particular trajectory are briefly summarized in the Wigner functions presented in Fig. 4a,b. Shown in Fig. 4a is an initial thermal state of the mechanical oscillator. After a period of continuous measurement of the AC component of , and in the presence of DC and thermal decoherence, this initially symmetric Gaussian state evolves into a nonGaussian bimodal quantum state, exhibiting Wigner negativity near the origin, as shown in Fig. 4b. See Supplementary Movie 1 for an animation of the Wigner function time evolution. Notably, qualitatively similar states have previously been shown to form in a different system under continuous positionsquared measurement and conditioning^{13}. The states prepared by our protocol exhibit many of the properties of the canonical Schrödinger cat state of Fig. 4c and are highly nonclassical. As a result, even in the presence of the identified decoherence mechanisms, we can conclude our protocol can give rise to interesting nonclassical states. We would like to highlight that initialization of the mechanical oscillator near its ground state is not required to generate nonclassical mechanical states. This insensitivity to initial thermal occupation is because the continuous positionsquared measurement also serves to purify the state. Further details of our simulation are found in Supplementary Note 10 and Supplementary Figs 7 and 8.
Discussion
To summarize, by exploiting the nonlinearity inherent in the radiationpressure interaction, we report nonlinear measurement of thermomechanical motion in an optomechanical system. Utilising the measurement of displacementsquared motion, we demonstrate the first measurementbased state preparation of mechanical nonGaussian states. Furthermore, we propose a method using feedback to extend this protocol to a quantum regime without requiring singlephoton strong coupling. Favourable scaling of the coupling rate in our approach makes realistic the possibility of observing the displacementsquared fluctuations at the level of the mechanical ground state in the near future. With sufficiently high detection efficiency, this would allow for mechanical quantum superposition state preparation. As a result, this experiment paves the way for quantum nonGaussian state preparation of mechanical motion via measurement with applicability to a number of other physical systems, such as cold atoms^{33}, atomic spin ensembles^{36}, optomechanical systems^{32} and superconducting microwave circuits^{31,34,37,38}.
Methods
Linear calibration procedure
We determine the evanescent optomechanical coupling by displacing the nanostring by a known distance using a piezoelectric element and measuring the resulting frequency shift on the optical resonance. The frequency shift is calibrated via modulation of known frequency applied to the laser. We then establish the response of the homodyne by sweeping the laser detuning over the optical resonance and measuring the slope of the phase response. This parameter combined with the previously determined optomechanical coupling rate gives the total response of the combined cavity interferometer system (V nm^{−1}), allowing direct calibration of the time domain data (nm). We calibrate the response of our spectrum analyser by applying a test tone of known amplitude, which using the time domain calibration gives a spectral peak of known displacement spectral density.
Quadratic calibration procedure
Frequency domain calibration of the quadratic measurement is performed by ensuring the calibrated RMS displacement, obtained from the linear measurement, which is consistent with the noise power of the 2ω_{M} peak, in accordance with the Isserlis–Wick theorem. In the time domain, a simple regression is used between the square of the linear measurement and the quadratic measurement . We verify that these procedures are consistent, to within known uncertainties, with one another and with the value of computed from the independently measured system parameters.
State conditioning
From the continuously acquired data, estimates of the quadratures at 2ω_{M} (ω_{M}) are obtained with the use of causal (acausal) decaying exponential filters, to time separate the conditioning and readout phases. From the filtered data at each discrete time step, we rotate the vector by an angle 2φ, such that a new vector is obtained. The simultaneously acquired linear data is then rotated through the half angle, φ, to obtain . For state preparation, the rotated linear data is conditioned on the value of , which is proportional to . We choose a conditioning window four times smaller than the quadratic measurement uncertainty. When the conditioning criterion is satisfied, the state is readout using the rotated linear data . All the data presented here have been generated from three 4 s blocks of sampled homodyne output.
Additional information
How to cite this article: Brawley, G. A. et al. Nonlinear optomechanical measurement of mechanical motion. Nat. Commun. 7:10988 doi: 10.1038/ncomms10988 (2016).
References
Deléglise, S. et al. Reconstruction of nonclassical cavity field states with snapshots of their decoherence. Nature 455, 510 (2008).
Ourjoumtsev, A., Jeong, H., TualleBrouri, R. & Grangier, P. Generation of optical Schrodinger cats from photon number states. Nature 448, 784 (2007).
Bimbard, E., Jain, N., MacRae, A. & Lvovsky, A. I. Quantumoptical state engineering up to the twophoton level. Nat. Photon. 4, 243–247 (2010).
Risté, D. et al. Deterministic entanglement of superconducting qubits by parity measurement and feedback. Nature 502, 350–354 (2013).
Knill, E., Laflamme, R. & Milburn, G. J. A scheme for efficient quantum computation with linear optics. Nature 409, 46–52 (2001).
Aspelmeyer, M., Kippenberg, T. J. & Marquardt, F. Cavity optomechanics. Rev. Mod. Phys. 86, 1391 (2014).
Vanner, M. R. et al. Pulsed quantum optomechanics. Proc. Natl Acad. Sci. USA 108, 16182–16187 (2011).
Vanner, M. R., Hofer, J., Cole, G. D. & Aspelmeyer, M. Coolingbymeasurement and mechanical state tomography via pulsed optomechanics. Nat. Commun. 4, 2295 (2013).
Szorkovszky, A. et al. Strong thermomechanical squeezing via weak measurement. Phys. Rev. Lett. 110, 183401 (2013).
Thompson, J. D. et al. Strong dispersive coupling of a highfinesse cavity to a micromechanical membrane. Nature 452, 72–75 (2008).
Miao, H., Danilishin, S., Corbitt, T. & Chen, Y. Standard quantum limit for probing mechanical energy quantization. Phys. Rev. Lett. 103, 100402 (2009).
Vanner, M. R. Selective linear or quadratic optomechanical coupling via measurement. Phys. Rev. X 1, 021011 (2011).
Jacobs, K., Tian, L. & Finn, J. Engineering superposition states and tailored probes for nanoresonators via openloop control. Phys. Rev. Lett. 102, 057208 (2009).
Ghirardi, G. C., Rimini, A. & Weber, T. Unified dynamics for microscopic and macroscopic systems. Phys. Rev. D 34, 470–491 (1986).
Diósi, L. Models for universal reduction of macroscopic quantum fluctuations. Phys. Rev. A 40, 1165–1174 (1989).
Penrose, R. On gravity’s role in quantum state reduction. Class. Quantum Gravity 28, 581–600 (1996).
Klecker, D. et al. Creating and verifying a quantum superposition in a microoptomechanical system. N. J. Phys. 10, 095020 (2008).
RomeroIsart, O. Quantum superposition of massive objects and collapse models. Phys. Rev. A 84, 052121 (2011).
Blencowe, M. P. Effective field theory approach to gravitationally induced decoherence. Phys. Rev. Lett. 111, 021302 (2013).
Børkje, K., Nunnenkamp, A., Teufel, J. D. & Girvin, S. M. Signatures of nonlinear cavity optomechanics in the weak coupling regime. Phys. Rev. Lett. 111, 053603 (2013).
Hudson, R. L. When is the wigner quasiprobability density nonnegative? Rep. Math. Phys. 6, 249–252 (1974).
Anetsberger, G. et al. Nearfield cavity optomechanics with nanomechanical oscillators. Nat. Phys. 5, 909–914 (2009).
Schmid, S., Jensen, K. D., Nielsen, K. H. & Boisen, A. Damping mechanisms in highQ micro and nanomechanical string resonators. Phys. Rev. B 84, 165307 (2011).
O’Connell, A. D. et al. Quantum ground state and singlephonon control of a mechanical resonator. Nature 464, 697–703 (2010).
Sankey, J. C., Yang, C., Zwickl, B. M., Jayich, A. M. & Harris, J. G. E. Strong and tunable nonlinear optomechanical coupling in a lowloss system. Nat. Phys. 6, 707–712 (2010).
FlowersJacobs, N. E. et al. Fibercavitybased optomechanical device. Appl. Phys. Lett. 101, 221109 (2012).
Purdy, T. P. et al. Tunable cavity optomechanics with ultracold atoms. Phys. Rev. Lett. 105, 133602 (2010).
Li, T., Kheifets, S. & Raizen, M. G. Millikelvin cooling of an optically trapped microsphere in vacuum. Nat. Phys. 7, 527 (2011).
Lin, Q., Rosenberg, J., Jiang, X., Vahala, K. J. & Painter, O. Mechanical oscillation and cooling actuated by the optical gradient force. Phys. Rev. Lett. 103, 103601 (2009).
Anetsberger, G. et al. Cavity optomechanics and cooling nanomechanical oscillators using microresonator enhanced evanescent nearfield coupling. Comptes Rendus Phys. 12, 800–816 (2011).
Teufel, J. D. et al. Sideband cooling of micromechanical motion to the quantum ground state. Nature 475, 359–363 (2011).
SafaviNaeini, A. H. et al. Squeezed light from a silicon micromechanical resonator. Nature 500, 185–189 (2013).
Brennecke, F., Ritter, S., Donner, T. & Esslinger, T. Cavity optomechanics with a BoseEinstein condensate. Science 322, 235–238 (2008).
Pirkkalainen, J.M. et al. Cavity optomechanics mediated by a quantum twolevel system. Nat. Commun. 6, 6981 (2015).
Macklin, C. et al. A near quantumlimited Josephson travelingwave parametric amplifier. Science 350, 307–310 (2015).
Hammerer, K., Sørensen, A. S. & Polzik, E. S. Quantum interface between light and atomic ensembles. Rev. Mod. Phys. 82, 1041 (2010).
Hatridge, M. et al. Quantum backaction of an individual variablestrength measurement. Science 339, 178–181 (2013).
Murch, K. W., Weber, S. J., Macklin, C. & Siddiqi, I. Observing single quantum trajectories of a superconducting quantum bit. Nature 502, 211–214 (2013).
Acknowledgements
We would like to thank K.E. Khosla, G.J. Milburn and T.M. Stace for useful discussion. This research was supported primarily by the ARC CoE for Engineered Quantum Systems (CE110001013). M.R.V. acknowledges support provided by an ARC Discovery Project (DP140101638). P.E.L., S.S. and A.B. acknowledge funding from the Villum Foundation VKR Centre of Excellence NAMEC (Contract No. 65286) and Young Investigator Programme (Project No. VKR023125).
Author information
Authors and Affiliations
Contributions
G.A.B. and M.R.V. contributed equally to this work. This quadratic measurement research programme was conceived by M.R.V. with refinements from G.A.B. and W.P.B. The optomechanical evanescent coupling setup was designed by G.A.B. and W.P.B. with later input from M.R.V. G.A.B. was the main driving force behind building the experiment and performing the data analysis with important input from M.R.V. and W.P.B. Microfabrication of the SiN nanostring mechanical resonators was performed by P.E.L., S.S. and A.B. This manuscript was written by M.R.V. and G.A.B. with important contributions from W.P.B. Overall laboratory leadership was provided by W.P.B. and substantial supervision for this project was performed by M.R.V.
Corresponding author
Ethics declarations
Competing interests
The authors declare no competing financial interests.
Supplementary information
Supplementary Information
Supplementary Figures 18, Supplementary Table 1, Supplementary Notes 111 and Supplementary References (PDF 2502 kb)
Supplementary Movie 1
Conditional dynamics of the mechanical state. (AVI 13111 kb)
Rights and permissions
This work is licensed under a Creative Commons Attribution 4.0 International License. The images or other third party material in this article are included in the article’s Creative Commons license, unless indicated otherwise in the credit line; if the material is not included under the Creative Commons license, users will need to obtain permission from the license holder to reproduce the material. To view a copy of this license, visit http://creativecommons.org/licenses/by/4.0/
About this article
Cite this article
Brawley, G., Vanner, M., Larsen, P. et al. Nonlinear optomechanical measurement of mechanical motion. Nat Commun 7, 10988 (2016). https://doi.org/10.1038/ncomms10988
Received:
Accepted:
Published:
DOI: https://doi.org/10.1038/ncomms10988
This article is cited by

Enhanced nonlinear optomechanics in a coupledmode photonic crystal device
Nature Communications (2023)

Nonlinearitymediated digitization and amplification in electromechanical phononcavity systems
Nature Communications (2022)

Tunable optical response in a hybrid quadratic optomechanical system coupled with single semiconductor quantum well
Quantum Information Processing (2022)

Optomechanical synchronization across multioctave frequency spans
Nature Communications (2021)

Nonclassical energy squeezing of a macroscopic mechanical oscillator
Nature Physics (2021)
Comments
By submitting a comment you agree to abide by our Terms and Community Guidelines. If you find something abusive or that does not comply with our terms or guidelines please flag it as inappropriate.