## Abstract

The periodicity inherent to any interferometric signal entails a fundamental trade-off between sensitivity and dynamic range of interferometry-based sensors. Here, we develop a methodology for substantially extending the dynamic range of such sensors without compromising their sensitivity, stability, and bandwidth. The scheme is based on simultaneous operation of two nearly identical interferometers, providing a moiré-like period much larger than 2π and benefiting from close-to-maximal sensitivity and from suppression of common-mode noise. The methodology is highly suited to atom interferometers, which offer record sensitivities in measuring gravito-inertial forces but suffer from limited dynamic range. We experimentally demonstrate an atom interferometer with a dynamic-range enhancement of more than an order of magnitude in a single shot and more than three orders of magnitude within a few shots for both static and dynamic signals. This approach can considerably improve the operation of interferometric sensors in challenging, uncertain, or rapidly varying conditions.

## INTRODUCTION

The ambiguity-free dynamic range of interferometric physical sensors is fundamentally limited to 2π radians. When the a priori phase uncertainty is larger than a single fringe, additional information is required to uniquely determine the physical quantity measured by the interferometer. If this quantity remains constant over long periods of time, then the phase ambiguity may be resolved through additional interferometric measurements with different scale factors, defined as the ratio between the interferometer phase and the magnitude of the physical quantity. A more challenging scenario arises when the physical quantity changes rapidly with time, and measurement with multiple scale factors must be realized simultaneously.

Overcoming this challenge in cold-atom interferometers (*1*), which have emerged over the past decades as extremely sensitive sensors of gravitational and inertial forces, is an especially ambitious proposition. Applications of atom interferometers vary from fundamental research (*2*–*6*) and precision measurements (*7*, *8*) to gravity surveys and inertial navigation (*9*). Mobile interferometers are being developed by several groups (*10*–*13*) with demonstrations of land-based, marine, and airborne gravity surveys (*14*–*16*).

In the latter applications, limited dynamic range is especially challenging, as the uncertainty in the acceleration to be measured is potentially very large. Reducing the interferometer scale factor or performing multiple measurements at each location results in reduced sensitivity or lower temporal bandwidth, respectively. A possible solution relies on auxiliary acceleration sensors with larger dynamic range but lower stability to constrain the interferometric measurement to a smaller, nonambiguous range (*17*, *18*). This hybrid approach has been previously used for mobile inertial measurements, e.g., on ships (*14*) and airplanes (*16*, *19*). However, it requires that the uncertainty in acceleration estimation from the auxiliary sensor be smaller than the 2π periodicity of the interferometric sensor. This may be difficult to achieve when operating the interferometer at maximum sensitivity owing to large variations in the auxiliary sensor bias, transfer function errors, misalignment between the sensors, or nonlinearities. Increasing the interferometer dynamic range beyond 2π would reduce sensitivity to such effects and enable hybrid operation under more challenging conditions. It is therefore highly desirable to have a high-sensitivity, high-bandwidth atom interferometer with a large dynamic range. While optical interferometers may gain such capabilities by using and detecting multiple wavelengths (*20*, *21*), this feat is more challenging for matter-wave interferometers.

In this work, we achieve a substantial enhancement of dynamic range on a single-shot basis by combining two powerful approaches in atom interferometry: increasing the dynamic range without sensitivity loss through small variations of the interferometer scale factor (*22*) and acquiring multiple phase measurements in a single experimental run (*23*, *24*). First, when the same fundamental physical quantity determines two interferometric phases with slightly different scale factors, it can be uniquely extracted within an enhanced dynamic range, determined by a moiré wavelength, which is inversely proportional to the difference between scale factors (Fig. 1A). Second, by operating and reading out the two interferometers simultaneously within the same experimental shot, major common-mode noises are efficiently rejected, increasing the scheme’s robustness to dominant sources of noise. In addition, such operation maintains the original temporal bandwidth of the measurement. Further exponential increase in dynamic range, at the cost of a linear reduction of temporal bandwidth, is achieved by varying the scale factor ratio between shots.

## RESULTS

### Principles of dual-*T* interferometry

We realize the above concept in a Mach-Zehnder atom interferometer measuring the local acceleration of gravity (*25*). Such devices use light pulses as “atom optics” that split the atomic wave packet into two arms and later recombine them after they traveled on macroscopically distinct trajectories. The differential phase accumulated between the arms of the interferometer depends on the motion of the atoms.

In our experiment, laser-cooled ^{87}Rb atoms are launched vertically on a free-fall trajectory. Counterpropagating, vertical laser beams at 780 nm drive two-photon Raman transitions between two electronic ground states while imparting recoil of two photon momenta (*26*). The Raman beams are sent from the top and are retro-reflected from a mechanically stabilized mirror at the bottom, which defines the reference frame with respect to which the motion of the atoms is measured. The interferometric sequence is composed of three Raman pulses, equally spaced by time *T*, acting to split the atomic wave packet into two components that drift apart, and then to redirect and recombine them, leading to a final atomic population ratio determined by the phase difference between the two arms.

In this configuration, the phase difference is determined by the gravitational acceleration *g* according to ϕ* _{a}* = (

*k*

_{eff}

*g*− α)

*T*

^{2}, with

*ℏk*

_{eff}as the total momentum transferred by the Raman interaction and α as a chirp rate applied to the relative frequency between the Raman beams to compensate for the changing Doppler shift of the falling atoms. Residual vibrations of the mirror contribute noise to the inertial phase ϕ

*.*

_{a}The concept we develop relies on a so-called dual-*T* operation of the interferometer. Instead of one pulse sequence, two interleaved pulse sequences with slightly different *T* values are performed (Fig. 1B). Raman transitions with counterpropagating beams are Doppler sensitive; that is, they efficiently address atoms only within a narrow distribution of vertical velocities. Therefore, by tuning the two-photon Doppler detuning of each set of pulses, one can independently address different velocity classes of the atoms (inset in Fig. 1B). We operate the two interferometers with scale factors differing by the ratio τ ≲ 1, choosing the interferometric durations *T*_{1} = *T* and *T* = 55 ms (see Materials and Methods).

Conventionally, the population ratio between the interfering atomic states is measured directly, and the cosine of the phase is extracted. In contrast, in our dual-*T* scheme, we detect the phases ϕ_{1}, ϕ_{2} of both interferometers by acquiring an image of the atoms in one of the final atomic states. We obtain the phase through phase shear readout (*27*), tilting the retro-reflecting Raman mirror by a small angle before the final π/2 pulses to add a horizontal phase gradient, and thereby generate a spatial transverse interference pattern across the cloud, as used in point-source interferometry (*28*–*30*). This detection method offers two advantages. First, the phase offset of the spatial interference pattern is directly extracted with constant sensitivity for all interferometric phases, in a manner equivalent to full quadrature detection, where both sine and cosine components of the phase are measured. Second, independent readout of both interferometers is inherently achieved owing to the mapping of the different velocity classes onto different vertical positions, due to ballistic expansion of the cloud. A typical image obtained in a single experiment is shown in Fig. 1C.

Figure 1D shows single-shot measurements in a dual-*T* operation with the dynamic range enhanced by a factor of 8. We vary ϕ* _{a}* by changing the chirp rate α with respect to its nominal value α

_{0}=

*k*

_{eff}

*g*, thereby emulating changes in

*g*. According to the equivalence principle, the scenario of the mirror being at rest with the lasers chirped at

*k*

_{eff}(

*g*−

*a*) and the scenario of the mirror accelerating at

*a*≠ 0 while the lasers are chirped at

*k*

_{eff}

*g*are indistinguishable from the point of view of the atoms. Varying the chirp rate is therefore the standard method to emulate changes in acceleration in a precise and controlled manner. We find that ϕ

*is mapped onto a unique set of straight, parallel lines in the plane spanned by ϕ*

_{a}_{1}and ϕ

_{2}owing to the quadrature detection capability. Conversely, conventional detection, which resolves only the cosine of the phase, would result in many phase ambiguities due to very different values of ϕ

*being mapped to similar measured phase components (Fig. 1E), severely limiting the benefits of a dual-*

_{a}*T*operation. Quadrature detection, together with the strong suppression of common noise due to operation at very similar scale factors, allows the dual-

*T*scheme to achieve a considerably larger enhancement compared to past implementations of simultaneous atom interferometers with different scale factors (

*23*).

### Phase estimation for single-shot dual-*T*

The measured interferometric phases ϕ_{1}, ϕ_{2} are constrained to the bare dynamic range ±π and can be written as

The integers *n*_{1} and *n*_{2}, which respectively bring ϕ_{1} and ϕ_{2} to the range ±π, are a priori unknown.

We define *D* ≡ (1 − τ)^{−1}, with τ = (*T*_{2}/*T*_{1})^{2} as the scale factor ratio. For integer values of *D*, the dynamic range enhancement is exactly *D*; as illustrated in Fig. 1A, ϕ_{1} and ϕ_{2} have a joint period of 2*D*π as in a moiré effect, resulting in an extended ambiguity-free dynamic range of ±*D*π (see Materials and Methods for discussion on noninteger values).

To analyze a dual-*T* measurement and extract an estimate for ϕ* _{a}*, we define the quantities ϕ

_{diff}and ϕ

_{sum}

ϕ_{diff} and ϕ_{sum} act as coarse and fine measurements, respectively. As shown in Fig. 2A, which presents an analysis of *D* = 8 dual-*T* measurements, ϕ_{diff} takes on a discrete set of 2*D* − 1 values. This constrain uniquely determines the values of *n*_{1} and *n*_{2} and hence the 2π subrange in which ϕ* _{a}* lies. Correspondingly, ϕ

_{sum}is a continuous variable, providing the estimation of the inertial phase ϕ

*within that subrange (see Materials and Methods).*

_{a}### Phase estimation for sequential operation

We now turn to discuss further enhancement of the dynamic range obtained by a sequence of several dual-*T* shots with alternating integer values of *D*. Here, we fix *T*_{1} and alternate *T*_{2} between shots. Assuming that changes in ϕ* _{a}* are smaller than π between consecutive shots, the above analysis per shot provides

*n*

_{1}mod

*D*. Together, the full sequence uniquely determines

*n*

_{1}within a range defined by the least common multiple of the used

*D*values, or, for coprime integers, simply their product (see Materials and Methods and fig. S1).

Analyses of two-shot operation with *D* = 7,8 and three-shot operation with *D* = 5,7,8 are shown in Fig. 2 (B and C). Each data point is a measurement with a random value of ϕ* _{a}* within the extended dynamic ranges ±56π and ±280π, respectively. We observe two- and three-dimensional clustering of the differential phases ϕ

_{diff}, where each cluster corresponds to a unique, nonambiguous phase range smaller than 2π.

### Noise and outlier probability

By virtue of simultaneously operating the two interferometers with similar scale factors, vibration-induced phase noise is highly correlated between them (Fig. 1F) and has negligible contribution to ϕ_{diff}. The dominant noise in ϕ_{diff} results from uncorrelated, independent detection noise in ϕ_{1} and ϕ_{2}, whose SD we denote as σ_{ind} (see Materials and Methods for a detailed discussion of noise terms).

As *D* is increased and the discrete values of ϕ_{diff} become denser, the uncorrelated noise may lead to errors in determining the correct subrange for ϕ* _{a}*, producing an outlier with phase estimation error in multiples of 2π. The probability ϵ for a measurement to be such an outlier is approximately (see Eq. 10 for exact expression)

Crucially, ϵ depends only on the uncorrelated noise and not on the vibration-dominated correlated noise, which is typically much larger. In the data presented in Fig. 2A, we observe one such outlier out of 5000 measurements for *D* = 8.

For the case of sequential dual-*T* operation, the total outlier probability depends on the outlier probabilities in each shot and, in the relevant regime of small error probabilities, is given simply by their sum. For any desired dynamic range and temporal bandwidth, the outlier probability is therefore minimized by choosing consecutive coprime values of *D*.

### Experimental performance

To quantify the performance of the dual-*T* scheme in terms of phase sensitivity and outlier probability, we extend the phase scan to random, known, values of ϕ* _{a}* within the range of ±1000π, corresponding to accelerations of ±65 mm/s

^{2}at

*T*= 55 ms. For each phase, we perform measurements with

*D*values between 5 and 15 and perform dual-

*T*analysis using each

*D*separately, using pairs of consecutive

*D*values, and using triplets of consecutive coprime

*D*values. We analyze each measurement within its appropriate extended dynamic range; data points that are outside the measurement’s relevant dynamic range are wrapped back onto it. We then compare the extracted phase to its expected value, from which we estimate the outlier probability ϵ as well as the phase residuals of the measurements without outliers.

The results, presented in Fig. 3, demonstrate an enhancement of dynamic range by factors of 10 in a single shot, ∼100 in two shots, and ∼1000 in three shots, while maintaining phase residuals of σ_{ϕ,est} ∼160 per shot (∼3.3 μm/s^{2} per shot), and with outlier probabilities of 0.5, 1.1, and 1.2%, respectively. In general, we find excellent agreement with the error model described in Eq. 4, with σ_{ind} = 80 mrad estimated from these data (see the Supplementary Materials).

We note that an outlier fraction on the order of 1% is acceptable in most applications, as such outliers can be identified and removed by comparison to adjacent shots or using auxiliary measurements. However, even if nearly zero outlier fraction is required, the dual-*T* scheme can deliver a substantial dynamic range enhancement. For example, with the above measured value of σ_{ind} and for *D* = 6, we expect ϵ ≈ 3 × 10^{−6}.

Furthermore, averaging over *N* repeated measurements with the same *D* value can decrease the outlier probability ϵ by effectively reducing σ_{ind} by a factor *D* as described above, the same value of ϵ may be achieved with considerably larger dynamic range enhancement, as seen from comparing solid and dashed curves in Fig. 3C.

### Stability of dual-*T* interferometry

To demonstrate the long-term stability of dual-*T* interferometry, we continuously measure gravity over 20 hours with *D* = 10. As shown in Fig. 4, ϕ* _{a}* follows the expected tidal gravity variations throughout the measurement period. It remains stable at time scales of 10

^{4}s to better than 100 nm/s

^{2}, consistent with past gravimetric measurements in our apparatus, showing that the dual-

*T*scheme does not add visible drifts to the estimated phase. Therefore, it is possible to reach the same accuracy as conventional interferometric operation relying on a one-off calibration run. Conversely, ϕ

_{diff}does exhibit small drifts, which we attribute to mutual light shift between the two interferometers. However, due to the discrete nature of ϕ

_{diff}, these drifts can be easily corrected in several ways (see Materials and Methods).

### Tracking fast-varying signals

We now turn to discuss dynamic scenarios, such as mobile gravity surveys or inertial measurements on a navigating platform, where the measured acceleration and thus ϕ* _{a}* change substantially between shots. Dual-

*T*interferometry with fixed

*D*can directly track a signal that randomly varies by up to ±

*D*π from shot to shot. Moreover, alternating the value of

*D*between consecutive measurements can enable tracking a signal with even larger variations; however, the sequential analysis described above cannot be applied due to the phase changing between shots, and a different analysis method is required.

To track such a signal, we use a particle filter estimation protocol (*31*, *32*). Particle filtering is a powerful and well-established technique in navigation science, signal processing, and machine learning, among other fields. It is a sequential, Monte Carlo estimation approach based on a large number of particles, which represent possible hypotheses of the system’s current state, e.g., the inertial phase measured by the sensor. These hypotheses are weighted through Bayesian estimation after every measurement, converging on a solution that is consistent with the sensor readings over time. In our context, under some model assumptions on the signal dynamics, use of particle filter enables full recovery of the single-shot bandwidth (*22*) while maintaining the large increase in dynamic range rendered by the sequential operation.

An experimental realization of tracking a dynamic signal is presented in Fig. 5. We change the chirp rate α between shots to simulate a band-limited random walk of *a* and perform dual-*T* measurements with alternating *D* = 9,10. The sequence of measured phases is then analyzed with a particle filter protocol using a second-order derivative model (see Materials and Methods) to extract best estimate for the time series of ϕ* _{a}*. Following a brief convergence period (fig. S6), we successfully track this time-varying signal, which spans over 2000π and changes by up to 40π between shots, with sensitivity per shot similar to measurements of static signals under similar conditions and with no outliers. We note that while the analysis was carried out in post-process, it is in principle compatible with implementation as a real-time protocol.

## DISCUSSION

In conclusion, we present an approach to atom interferometry for substantial enhancement of dynamic range without compromising sensitivity and measurement bandwidth. In applications where traditional atom interferometers must be operated at reduced sensitivity owing to the expected dynamic range of the measured signal, our approach enables measurements with a substantial increase in sensitivity while maintaining the necessary dynamic range.

Taking advantage of full-quadrature phase detection and common-noise rejection, we experimentally demonstrate an increase of dynamic range by more than an order of magnitude in a single shot. Incorporating data from several consecutive shots, the dynamic range further increases in exponential fashion, allowing us to reach three orders of magnitude gain using only three measurements. Last, we demonstrate tracking of a dynamical signal with tens of radians shot-to-shot variation by combining the dual-*T* measurement with a particle filter protocol, representing a major improvement compared to recent works (*22*).

This approach can considerably enhance performance of sensors and, in particular, inertial-sensing atom interferometers, under challenging conditions, by enabling nonambiguous operation without sacrificing either sensitivity or bandwidth. Such conditions are encountered in field operation of such sensors, for example, in mobile gravity surveys or when used for inertial navigation on a moving platform. By extending the sensor real-time dynamic range, the requirements on vibration isolation or corrections based on auxiliary measurements can be relaxed or, equivalently, existing sensors can be operated in more demanding environments at higher sensitivities. Therefore, it complements and potentially improves the technique of hybridization with a classical sensor.

Dual-*T* measurements can be realized by multiple means, based on known atom interferometry tools, e.g., dual-species interferometry (*23*) or momentum-state multiplexing (*24*), in addition to phase shear readout (*27*) used in this work. It is also compatible with important atom interferometry practices, such as *k*-reversal (*33*, *34*) and zero–dead-time operation (*35*). Further improvement of the scheme is possible by incorporating more than two interferometric sequences within the same experimental shot, enabling the gain demonstrated here for sequential operation within a single shot. The dual-*T* approach may also be applied in other atom interferometers, such as gyroscopes in the butterfly configuration (*36*, *37*) and multiaxis inertial sensors in launched (*38*, *39*) or continuous (*40*) configurations.

## MATERIALS AND METHODS

### Details of the experiment

We load a cloud of ^{87}Rb atoms in a magneto-optical trap (MOT) and launch it upward at 0.9 m/s with moving optical molasses, which also cools the cloud to 5 μK. Atoms initially populate equally all *m _{F}* sublevels in the

*F*= 2 hyperfine manifold. We select atoms in two distinct velocity classes and in the

*m*= 0 state using two counterpropagating Raman π pulses, with 20-μs duration and a relative Doppler detuning of 80 kHz. Two interferometric sequences of π/2 − π − π/2 pulses, with durations of 12, 24, and 12 μs, respectively, address each of the velocity classes as shown in Fig. 1. The timing of the π pulses of the two interferometers is set to 22 and 22.5 ms after the apex of the trajectories. The precise ratio of

_{F}*T*

_{2}/

*T*

_{1}contains empirically calibrated corrections on the order of 10

^{−5}with respect to the naïve

*41*). Before the final π/2 pulses, the Raman mirror is tilted by 120 μrad. With the MOT beams tuned on resonance with the

*F*= 2 →

*F*= 3 cycling transition, a fluorescence image of atoms in the

*F*= 2 level is taken on a charge-coupled device camera oriented perpendicularly to the Raman mirror tilt axis. The experiment is repeated every 2 to 3 s.

### Extraction of the measured phases ϕ_{1}, ϕ_{2}

We first integrate the image horizontally to find the vertical Gaussian envelopes of the fringe patterns, which are used to define the analysis region of interest for each interferometer (fig. S2). We then vertically integrate the image over those regions and fit the resulting profile to Gaussian envelopes with sinusoidal modulation. The phases of the measurement are taken as the phases of the fitted fringes at the horizontal center of the cloud. Last, we calculate and correct the vibration-induced phase based on the auxiliary accelerometer signal (Nanometrics Titan), taking into account the different interrogation times of each interferometer.

### Single-shot dual-*T* analysis

For each dual-*T* shot, we rotate the measured ϕ_{1}, ϕ_{2} according to Eq. 3

Within the extended dynamic range of ±*D*π for ϕ* _{a}*, the integer

*n*

_{1}takes values within ±⌊

*D*/2⌋, and Δ

*n*=

*n*

_{1}−

*n*

_{2}takes either 0 or ± 1. From ϕ

_{diff}, we uniquely determine Δ

*n*

*n*

_{1}follows as the round value of

*D*[(1 + τ

^{2})ϕ

_{diff}/(2π) + Δ

*n*]. Last, we estimate ϕ

*by substituting*

_{a}*n*

_{1}and

*n*

_{2}=

*n*

_{1}− Δ

*n*back into ϕ

_{sum}.

All measurements presented in this work were performed in a noisy urban-industrial environment and include passive vibration isolation and postprocessing correction of residual vibrations using the auxiliary accelerometer. The residual vibration phase noise is usually reduced to at most 200 mrad and post-processing correction of residual vibrations using the auxiliary accelerometer. By calculating the vibration-induced phase for each of the two interferometers based on their individual transfer function (*42*), the residual vibration phase noise is reduced to at most 300 mrad and typically below 200 mrad. However, as demonstrated in fig. S3, the dual-*T* approach works equally well also for substantially larger vibration noise (e.g., without correction based on the auxiliary accelerometer).

We focused the discussion on integer *D*. Rational *D* yields joint phase periodicity according to the lowest term numerator of *D* but with less efficient common-mode noise rejection. For irrational *D*, there is no well-defined periodicity and hence no discrete set of allowed ϕ_{diff} solutions. While, in both cases, dynamic range enhancement is attained, optimal results are achieved for integer *D*.

### Sequential dual-*T* analysis

From a sequence of *N* (*N* = 2,3 in this work) shots with alternating *D*^{(i)}, where *i* = 1, …, *N*, we retrieve *N* pairs of phases *D*^{(i)}/2⌋. Joint analysis of the sequential measurements in principle amounts to finding the integer *n*_{1} that satisfies the set of equations *D*^{(1)}, …, *D*^{(N)}), LCM denoting the least common multiple. This analysis assumes that *i*, as the first interferometer always measures ϕ* _{a}* with the same interrogation time

*T*. However, for values of ϕ

*close to odd multiples of π, phase noise may cause variations of up to ±1 in*

_{a}*i*> 1 as the round value of

*n*

_{1}. This estimation of

*does not change by more than π between shots, setting the limit for allowed ϕ*

_{a}*variations for sequential dual-*

_{a}*T*analysis. In Fig. 2B, only measurements with

### Experimental noise parameterization

Extending on Eqs. 1 and 2, we write the phases ϕ_{1}, ϕ_{2} as

Here, _{corr} and δϕ_{ind} as vibration noise and detection noise, respectively, this correspondence is not complete. For example, vibrations at higher frequencies, for which the transfer functions of the two interferometers differ, would contribute to the estimate of the independent noise.

With this parameterization and based on Eq. 3, ϕ_{diff} and ϕ_{sum} are characterized by random noise with SDs _{diff} from its theoretical value is larger than half the difference between its discrete solutions, which is 2π/[*D*(1 + τ^{2})]. The probability of such an event is given by

### Systematic phase shifts

Dual-*T* measurements have several systematic phase shifts that are common also to conventional atom interferometers, due to factors such as one-photon light shifts, two-photon light shifts (*43*), and offset of the Raman frequency from Doppler resonance (*44*). Typically, either these effects are estimated and accounted for theoretically or they are eliminated through wave vector reversal (*k*-reversal) (*33*, *34*).

Nevertheless, some of these shifts may be complicated or modified by the existence of two simultaneous interferometer pulse sequences, while new sources of systematic shifts may arise, such as due to an estimation error of the cloud center position when using phase shear readout. As demonstrated in Fig. 4, these effects do not contribute to bias instability in the measured phase up to few milliradians, although they may introduce a constant bias, which can be determined and calibrated in advance by comparison of dual-*T* measurements with standard interferometry. We correct this bias by performing 15 to 50 initial calibration measurements for different *D* values and *k*_{eff} signs, where we assume prior knowledge of ϕ* _{a}*. For the time-varying experiment in Fig. 5, these calibration measurements are not included in the particle filter analysis.

### Correction of drifts in the differential phase

As shown in fig. S5A, ϕ_{diff} exhibits small drifts over time from its expected discrete value. While these drifts do not directly enter into the estimation of ϕ* _{a}*, they may have a large impact on outlier probability ϵ. By performing

*k*-reversal, we observe that the drift in ϕ

_{diff}is antisymmetric with respect to

*k*

_{eff}. We therefore attribute the observed phase drifts to differential light shift between the two interferometric states of the Raman pulses. As the temporal response function to external phase shifts is antisymmetric with respect to the central π pulse, normally, the effect of light shifts due to the interferometer pulses cancels up to changes in the light shift during the interferometer due to laser intensity fluctuations (

*45*). In our dual-

*T*realization, the light shift induced by the π/2 pulses of the shorter interferometer on the longer one still cancels as before, but each interferometer experiences an uncompensated light shift owing to the π pulse of its counterpart. A realization of dual-

*T*with simultaneous π pulses for both interferometers will circumvent this effect (

*23*).

These mutual light shifts will be of approximately equal amplitude but opposite signs; therefore, they are suppressed in ϕ_{sum} by a factor (1 − τ)/(1 + τ^{2}) but amplified in ϕ_{diff} by a factor (1 + τ)/(1 + τ^{2}). These effects of light shifts are entirely canceled by performing *k*-reversal, and, as we observe in fig. S5B, the average value of ϕ_{diff} over ±*k*_{eff} remains stable at time scales of 10^{4} s to better than 1 mrad. In the particle filter demonstration, we used both *k*_{eff} signs to correct such drifts, demonstrating the compatibility of the *k*-reversal technique with the dual-*T* approach.

In addition, because of the discrete nature of ϕ_{diff}, the observed drifts can also be deterministically corrected without requiring *k*-reversal and thus with practically no impact on the interferometer performance or bandwidth. For the data presented in Figs. 2 and 3, we continuously correct drifts in ϕ_{diff}, without assuming prior knowledge of ϕ* _{a}*, by tracking the difference between the measured ϕ

_{diff}values from the nearest discrete values and subtracting their long-term, moving average.

### Particle filter implementation

We choose as state variables the instantaneous value of the inertial phase ϕ* _{a}* and its first- and second-order time derivatives, denoting

*m*th particle at the

*i*th time step. As observables, we choose the two interferometer phases ϕ

_{1,2}. The initial value and derivatives of the input ϕ

*signal are approximately −207π, 8.6π/*

_{a}*dt*, and 4.5π/

*dt*

^{2}, respectively. We represent a scenario where some imperfect knowledge about the starting conditions exists by drawing the initial values of the particles from normal distributions characterized by

At each time step of the filter, we first propagate the particles’ state according to *x*^{(m,i + 1)} = **F** · *x*^{(m,i)} + *w*^{(m,i)}, with **F** being the state propagation matrix and *w*^{(m,i)} being a random process noise with zero mean and covariance matrix **Q**. For our model, we have*dt* is the time interval between consecutive measurements. Following state propagation, we calculate the expected interferometer signals for each particle as ^{(i)} is the scale factor ratio in the *i*th measurement. We calculate their residuals from the actual measurements modulo 2π and weigh each particle according to the likelihood that these residuals are consistent with the independent measurement noise σ_{ind}, which we take as 73 mrad according to the spread of δϕ_{ind,diff}. State variable estimation is achieved by using a ridge-detection algorithm (MATLAB tfridge function) on the time-dependent particle histogram to estimate *dt*^{2}, as it minimizes the mean error of the estimated ϕ* _{a}* from the measured ϕ

_{1,2}.

## SUPPLEMENTARY MATERIALS

Supplementary material for this article is available at http://advances.sciencemag.org/cgi/content/full/6/45/eabd0650/DC1

This is an open-access article distributed under the terms of the Creative Commons Attribution-NonCommercial license, which permits use, distribution, and reproduction in any medium, so long as the resultant use is **not** for commercial advantage and provided the original work is properly cited.

## REFERENCES AND NOTES

**Acknowledgments:**

**Funding:**This work was supported by the Pazy Foundation, the Israel Science Foundation, and the Consortium for quantum sensing of Israel Innovation Authority.

**Author contributions:**D.Y. and C.A. built the apparatus, performed the measurements, and analyzed the data. N.D. and O.F. supervised the research. All authors contributed to the writing of the manuscript.

**Competing interests:**The authors declare that they have no competing interests.

**Data and materials availability:**All data needed to evaluate the conclusions in the paper are present in the paper and/or the Supplementary Materials. Additional data related to this paper may be requested from the authors.

- Copyright © 2020 The Authors, some rights reserved; exclusive licensee American Association for the Advancement of Science. No claim to original U.S. Government Works. Distributed under a Creative Commons Attribution NonCommercial License 4.0 (CC BY-NC).