## Abstract

Nanomechanical devices have attracted the interest of a growing interdisciplinary research community, since they can be used as highly sensitive transducers for various physical quantities. Exquisite control over these systems facilitates experiments on the foundations of physics. Here, we demonstrate that an optically trapped silicon nanorod, set into rotation at MHz frequencies, can be locked to an external clock, transducing the properties of the time standard to the rod’s motion with a remarkable frequency stability *f*
_{r}/Δ*f*
_{r} of 7.7 × 10^{11}. While the dynamics of this periodically driven rotor generally can be chaotic, we derive and verify that stable limit cycles exist over a surprisingly wide parameter range. This robustness should enable, in principle, measurements of external torques with sensitivities better than 0.25 zNm, even at room temperature. We show that in a dilute gas, real-time phase measurements on the locked nanorod transduce pressure values with a sensitivity of 0.3%.

## Introduction

Frequency is the most precisely measured quantity in physics, and stable oscillators have found a plethora of applications in metrology. While pendulum clocks exploited the stability of mechanical motion to keep track of time, state-of-the-art atomic clocks rely on well-defined internal resonances of atoms, achieving a precision of a few parts in 10^{18} (ref. ^{1}). To exploit the stability of clocks for physical applications, it is essential to develop “gearboxes” that can be synchronized to a good time standard, translating atomic definiteness into other domains of physics. Phase-locked quartz oscillators^{2} and frequency combs are examples of such transducers, imprinting clock stability onto a mechanical system or light field respectively, with high accuracy^{3}.

Nano- and micromechanical systems are of great technological interest, due to their low mass and extreme sensitivity to external forces^{4,5,6}, torques^{7, 8}, acceleration^{9}, displacement^{10, 11}, charge^{12}, and added mass^{13, 14}. Many of these systems are themselves realizations of harmonic oscillators, with frequency stabilities reaching *f*/Δ*f* = 10^{8} (refs. ^{15, 16}), which can be further improved through mechanical engineering^{17}, injection locking^{18, 19}, electronic feedback^{20}, or parametric driving^{21}. The contact-free mechanical motion of particles suspended by external fields in vacuum^{22,23,24,25,26,27,28,29} can reach a frequency stability that is only limited by laser power fluctuations and collisional damping by residual gas particles^{30}.

In this work, we transduce clock stability into the rotation of an optically trapped silicon nanorod in vacuum. By periodically driving the rotation with circularly polarized light, we create a nanomechanical rotor whose rotation frequency *f*
_{r}, and frequency noise, is determined by the periodic drive alone. This driven rotor is sensitive to non-conservative forces, and the operating frequency can be tuned by almost 10^{12} times its linewidth. Through our method, the frequency stability is independent of material stress, laser noise, and collisional damping. The driven nanorotor operates at room temperature, and across a wide pressure range from low vacuum to medium vacuum, achieving a pressure resolution of three parts-per-thousand, and in principle allowing a torque sensitivity below the zepto-Nm level.

## Results

### Frequency locking

We levitate a nanofabricated silicon nanorod in the standing light wave formed by two counterpropagating laser beams, and track its motion by monitoring the scattered light, see Fig. 1a and “Methods”. When the laser is linearly polarized, the nanorod is harmonically trapped in an antinode of the standing wave and aligned with the field polarization. When the laser is circularly polarized, the scattered light exerts a torque^{29, 31, 32} and propels the nanorod in the plane orthogonal to the beam axis, while its center-of-mass remains trapped^{29}. The maximum rotation frequency of the rod is determined by its size, the pressure, and the laser intensity^{29}. Collisions with gas particles, and center-of-mass excursions into regions of different light intensity, give rise to a broad distribution of rotational frequencies^{29}, as shown by the blue curve in Fig. 1c.

However, if the rod is driven by periodically switching the laser polarization between linear and circular, the rod can frequency lock to this modulation, leading to a sharp peak in the power spectral density (PSD) of the scattered light (Fig. 1b). The locked rotation peak is eleven orders of magnitude narrower than in the unlocked case (Fig. 1c). The rotation frequency can be continuously tuned over a range of 10^{12} linewidths whilst locked to the periodic drive, retaining its high frequency stability.

In order to characterize the frequency-locked rotation, we drive the nanorod with frequency *f*
_{d} = 1.11 MHz, at a gas pressure *p*
_{g} = 4 mbar and total laser power *P* = 1.35 W. We record its motion continuously for four days (see “Methods” section). The PSD of the locked rotation is shown in Fig. 1b. We record an extremely narrow feature, which yields a Lorentzian FWHM below 1.3 μHz within one standard deviation. In this way, we achieve rotational stability with a phase noise −80 dBc Hz^{−1} below the signal at only 3 mHz from the carrier frequency (Fig. 2).

### Stable limit cycles

To explain this ultra-stable rotation, we model the dynamics of the rod’s orientation *α* with respect to the polarization axis^{29}. Denoting by Γ the damping rate due to gas collisions (a function of gas pressure *p*
_{g}), by *N* the torque exerted by the circularly polarized standing wave (a function of laser power *P*) and by *V* the maximum potential energy of the rod in a linearly polarized standing wave, the equation of motion is

where \(I = M\ell ^2{\mathrm{/}}12\) is the moment of inertia and *h*(*t*) represents the periodic driving, with *h*(*t*) = 1 for circular polarization at *t* ∈ [0, 1/2*f*
_{d}) and *h*(*t*) = 0 for linear polarization at *t* ∈ [1/2*f*
_{d}, 1/*f*
_{d}); expressions for Γ, *N*, and *V* are given in “Methods” section.

In the limit of long driving times \(t \gg 1{\mathrm{/}}f_{\mathrm{d}}\) the nanorod rotates with constant mean rotation frequency \(f_{\mathrm{r}} = \left\langle {\dot \alpha } \right\rangle {\mathrm{/}}2\pi\), and its motion approaches one of two qualitatively distinct types of limit cycles. In the first type, threshold rotation, *f*
_{r} = *N*/(4*πI*Γ) is determined by the balance between Γ and the time averaged radiation torque *N*/2. Threshold rotation exhibits a broad frequency distribution, as shown by the blue curve in Fig. 1c, due to its dependence on *P* and *p*
_{g}
^{29}. It should be noted, that the behavior of threshold rotation is almost identical to illuminating the nanorotor continuously with circularly polarized light, which propels the rod at a maximum rotation frequency *f*
_{r} = *N*/(2*πI*Γ).

In the second type of limit cycle, the aforementioned locked rotation, *f*
_{r} locks to a rational fraction of the driving frequency. Experimentally, we observe *f*
_{r}:*f*
_{d} = 1:2– and *f*
_{r}:*f*
_{d} = 1:4–locking, where the rod performs one rotation in two or four driving periods, respectively. The rotational frequency *f*
_{r} now does not depend on environmental parameters such as *p*
_{g} or *P*, but only on the frequency stability of the drive. Locked rotation is shown in Fig. 1b and the red curve in Fig. 1c.

The realized limit cycle is determined by the initial dynamics of the nanorod, and by experimental parameters such as *p*
_{g}, *P*, *f*
_{d}, and the rod dimensions. For a given nanorod the ratio between torque and potential is fixed, and thus Eq. (1) depends only on the dimensionless damping rate Γ/*f*
_{d} and dimensionless torque \(N{\mathrm{/}}f_{\mathrm{d}}^2I\). In Fig. 3a we show this reduced parameter space. The blue shaded area indicates the region where 1:2–locking is possible. The labeled solid lines indicate where threshold and locked rotations have the same frequency, and locking occurs independent of the initial conditions.

### Rotational dynamics

To explore the dynamics of the driven nanorotor, we experimentally vary *p*
_{g} and *f*
_{d}, thereby following a path through parameter space (red line in Fig. 3a). The observed *f*
_{r} are shown as blue points in Fig. 3b, the top panel showing the path 1–2–3, and the lower panels 3–4. This plot shows that for certain parameters both types of limit cycles can be observed, depending on the initial conditions. When starting from 1, the rotation 1:2–locks to the drive (horizontal solid line). When increasing *p*
_{g} along 1–2, the rod jumps out of lock, and exhibits threshold rotation. When decreasing *f*
_{d} along 2–3, the rod remains at threshold rotation, following the theoretically expected frequencies with excellent agreement (orange dotted lines). Decreasing *p*
_{g} along 3–4, the rod first follows the threshold rotation frequency until it crosses the horizontal line, where it briefly enters 1:4–locked rotation, returns to threshold rotation and eventually jumps into 1:2–locked rotation. The solid red lines in Fig. 3b are the theoretically predicted *f*
_{r} for an adiabatic path through parameter space, with the discrepancy due to imperfect adiabatic control in the experiment.

### Applications

For 1:2–locked rotation, the phase lag *ϕ* between the drive and the rotation is

it depends upon gas pressure *p*
_{g} through Γ and on laser power *P* through *V* and *N*. The requirement that this phase is real defines the shaded region in Fig. 3a. The phase *ϕ* is sensitive to non-conservative forces, such as light or gas scattering.

A lock-in amplifier is used to monitor *ϕ* (see “Methods” section), yielding real-time readout of phase variations. For a constant laser power *P*, measuring the phase amounts to local sensing of the gas pressure *p*
_{g}, as shown in Fig. 4b. We achieve a relative pressure sensitivity of 0.3%, which is currently limited only by the intensity noise of the fiber amplifier. This sensitivity may still be improved by five to six orders of magnitude by stabilizing the power^{33}. This shows the great potential of our system as a pressure sensor. The fine spatial resolution provided by the micrometer-sized rotor could allow, for instance, mapping of velocity fields and turbulences in rarefied gas flows or atomic beams.

The driven nanorod is sensitive to externally applied torques through Eq. (1). In analogy to the pressure sensing application, the phase between the drive and the driven rotation of the locked rotor provides a real-time readout with a bandwidth of 100 kHz set by the lock-in amplifier. From Eq. (2), the torque sensitivity can be estimated as 2.4 × 10^{−22} Nm for our current experimental parameters, which at room temperature would be the highest value achieved in state of the art systems^{8}, and which could also be significantly improved by laser power stabilization. This sensitivity can be reached for any non-conservative force, that varies on a timescale longer than 1/*f*
_{d}. The bandwidth and sensitivity of this sensor for arbitrary torques warrants further investigation.

## Discussion

In conclusion, we have presented a technique for locking the rotation of a levitated nanomechanical rotor to a stable frequency reference, leading to a high mechanical frequency stability which can be used for instantaneous, highly sensitive local measurements of pressure or torque. One great advantage of the locked nanorotor over nanomechanical resonators is the absence of an intrinsic resonance frequency. By varying *f*
_{d} we can tune the rotation frequency over almost 10^{12} linewidths while retaining its stability, as shown in Fig. 4a, circumventing the low bandwidth that naturally comes with highly sensitive resonant detectors. Measuring a phase lag rather than a frequency shift allows us to monitor force variations in real time, bypassing the inherent growth in measurement time that comes with decreasing linewidth in a resonant sensor.

Our system is sensitive to non-conservative forces, such as those due to photon absorption or emission, shear forces in gas flows, radiation pressures in light fields, optical potentials, mass and size variations of the rod due to gas accommodation, and local pressure and temperature variations in the gas. Employing higher optical powers, larger duty cycles of the drive, or lower gas pressures will increase the sensing range by a factor of more than ten, while retaining the exquisite sensitivity. The stability of the locked nanorotor may be further increased by driving it with a more stable clock. By reaching ultra high vacuum, this technique may also be suited to prepare quantum coherent rotational dynamics^{34}, for which the high frequency stability may be exploited.

## Methods

### Nanorod trapping

A silicon nanorod of length \(\ell = \left( {725 \pm 15} \right)\) nm and diameter *d* = (130 ± 13) nm (with mass *M* = 2.2 × 10^{−17} kg) is trapped at a pressure of *p*
_{g} = 4 mbar, using light of total power *P* = 1.35 W with RMS power fluctuations of 0.3%. Our method of producing and trapping the nanorods is described in refs. ^{29, 35}. The motion is monitored by placing a 1 mm core multimode fiber less than 100 μm from the trapped nanorod, which collects the light that the nanoparticle scatters, yielding information about all translational and rotational degrees of freedom.

### Rotation analysis

In order to record a time series as long as 4 days we mix down the scattered light with a local oscillator at frequency *f*
_{LO} such that the rotational motion signal of the rod is shifted to a frequency of 190 Hz (Fig. 1a) and digitized with a sampling rate of 2 kS s^{−1}. This signal can then be used to calculate the phase noise \(S_\phi (f) = 10\,{\mathrm{log}}_{10}\left[ {{\mathrm{PSD}}(f){\mathrm{/PSD}}\left( {f_{\mathrm{d}}} \right)} \right]\) in units of dBc Hz^{−1}. The drive signal is recorded and analyzed in the same way.

To extract the relative phase *ϕ* of the nanorod rotation with respect to the drive we use a Stanford Research Systems lock-in amplifier (SR830) which performs a homodyne measurement on the mixed-down 190 Hz scattering signal. For this purpose both the modulation frequency *f*
_{d} and the local oscillator *f*
_{LO} are synced to a common clock.

### Rotational dynamics

The rotational motion depends crucially on the damping rate Γ, the radiation torque *N*, and the laser potential *V*, through Eq. (1). All three quantities can be evaluated microscopically as detailed in refs. ^{29, 36}. Specifically, the rotational damping rate due to diffuse reflection of gas atoms with mass *m*
_{g}, evaluated in the free molecular regime, is \(\Gamma = d\ell p_{\mathrm{g}}\sqrt {2\pi m_{\mathrm{g}}} (6 + \pi ){\mathrm{/}}8M\sqrt {k_{\mathrm{B}}T}\), where *T* denotes the gas temperature. The optical torque exerted by a circularly polarized standing wave can be evaluated by approximating the internal polarization field according to the generalized Rayleigh–Gans approximation^{36} as \(N = P\Delta \chi \ell ^2d^4k^3\left[ {\Delta \chi \eta _1(k\ell ) + \chi _ \bot \eta _2(k\ell )} \right]{\mathrm{/}}48cw_0^2\), where *k* = 2*π*/*λ* is the wavenumber, \(\Delta \chi = \chi _{||} - \chi _ \bot\) depends on the two independent components of the susceptibility tensor and \(\eta _1(k\ell ) = 0.872\) and \(\eta _2(k\ell ) = 0.113\)
^{29}. In a similar fashion, one obtains for the laser potential \(V = Pd^2\ell \Delta \chi {\mathrm{/}}2cw_0^2\).

The phase lag (2) is obtained by averaging the equation of motion (1) over one driving period 1/*f*
_{d} and exploiting that the motion is 1:2-locked, \(\left\langle {\dot \alpha } \right\rangle = \pi f_{\mathrm{d}}\) while \(\left\langle {\ddot \alpha } \right\rangle = 0\) and, consequently, *α*(*t*) = *α*
_{0} + *πf*
_{d}
*t*. The phase difference between the polarization change from circular to linear and the maximum scattering signal observed when the rod is oriented orthogonal to the detector (*α*(*t*) = *π*) is *ϕ* = *π* − 2*α*
_{0} leading to Eq. (2).

### Data availability

All relevant data are available from the corresponding author upon request.

## Additional information

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## Acknowledgements

We are grateful for financial support by the Austrian Science Fund (FWF) in the projects P27297 and DK-CoQuS (W1210). We acknowledge support by S. Puchegger and the faculty center for nanostructure research at the University of Vienna in imaging the nanorods. J.M. acknowledges funding from the European Unions Horizon 2020 research and innovation program under the Marie Skłodowska-Curie grant agreement no. 654532. F.P. acknowledges the Legacy Program (Israel Science Foundation) for its support.

## Author information

### Affiliations

#### University of Vienna, Faculty of Physics, VCQ, Boltzmanngasse 5, 1090, Vienna, Austria

- Stefan Kuhn
- , Markus Arndt
- & James Millen

#### University of Duisburg-Essen, Lotharstraße 1, 47048, Duisburg, Germany

- Benjamin A. Stickler
- & Klaus Hornberger

#### School of Chemistry, Tel-Aviv University, Ramat-Aviv, 69978, Israel

- Alon Kosloff
- & Fernando Patolsky

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### Contributions

S.K., M.A. and J.M. conceived of and designed the experiment. S.K. and J.M. performed all experiments. S.K., B.A.S. and J.M. analyzed the data. A.K. and F.P. fabricated the nanorods. B.A.S. and K.H. developed all theoretical models. S.K., B.A.S., K.H., M.A. and J.M. contributed to the writing of the manuscript.

### Competing interests

Aspects of this work are subject to a filed patent application.

### Corresponding author

Correspondence to Stefan Kuhn.

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