## Abstract

An SU(1,1) interferometer, which replaces the beam splitters in a Mach–Zehnder interferometer with nonlinear interactions, offers the potential of achieving improved phase sensitivity in applications with low optical powers. We present a novel variation on the SU(1,1) interferometer in which the second nonlinear interaction is replaced with balanced homodyne detection. We show theoretically that this “truncated SU(1,1) interferometer” can achieve the same potential phase sensitivity as the conventional SU(1,1) interferometer. We build an experimental realization of this device using seeded four-wave mixing in ${}^{85}\mathrm{Rb}$ vapor as the nonlinear interaction, thus employing a bright two-mode squeezed state as the phase-sensing quantum state inside the interferometer. Measurements as a function of operating point show that even with $\approx 35\%$ loss, this device can surpass the standard quantum limit by 4 dB. This device is simpler to build and operate than the conventional SU(1,1) interferometer, and also eliminates some sources of loss, thus making it useful for applications in precision metrology.

© 2017 Optical Society of America

## 1. INTRODUCTION

Precision phase measurements are invaluable for a wide range of applications, including gravitational wave detection and biological sensing [1–3]. The sensitivity of phase-measuring devices, such as interferometers, is characterized by the uncertainty of a single phase measurement $\mathrm{\Delta}\varphi $. When using coherent optical fields in a Mach–Zehnder interferometer, the phase sensitivity is bounded by the standard quantum limit (SQL) $\mathrm{\Delta}\varphi =1/\sqrt{N}$, where $N$ is the mean photon number in a single phase measurement.

The phase sensitivity of an interferometer can be improved by using quantum resources [3–5]. By injecting squeezed states [6–8] or other nonclassical states [3,9–11] into a conventional Mach–Zehnder interferometer, for example, one can achieve phase sensitivities that surpass the SQL.

An alternative to injecting quantum states into a Mach–Zehnder interferometer is to replace the passive beam splitters in such a device with active nonlinear optical elements [12]. A particular configuration that has drawn considerable interest is the SU(1,1) interferometer [12], which is expected to achieve phase sensitivities beyond the SQL even in the presence of loss [13–16]. The SU(1,1) interferometer takes two input modes and, using parametric down-conversion or four-wave mixing (4WM), produces a two-mode squeezed state that is used for phase sensing, as shown in Fig. 1. We consider the seeded version of the SU(1,1) interferometer, where the phase-sensing two-mode state consists of two bright beams. These beams are then recombined in another nonlinear process, and any changes in the phase sum of the two modes relative to the pump phase can be inferred by detecting the light at the outputs, either by using homodyne detection or direct intensity detection.

We present a variation on the SU(1,1) interferometer that replaces the detection schemes shown in Fig. 1(a), including the second nonlinear interaction, with the simpler arrangement shown in Fig. 1(b). This scheme eliminates losses associated with the second nonlinear process, such as imperfect mode matching of the beams and absorption in the medium. We show theoretically that the phase-sensing ability of this seeded “truncated SU(1,1) interferometer” is the same as that of the full SU(1,1) interferometer shown in Fig. 1(a) (i) and surpasses the sensitivity of the direct-detection schemes shown in Fig. 1(a) (iii, iv). We build a version of the truncated SU(1,1) interferometer using 4WM and show how the potential phase sensitivity of this device beats the SQL over a range of operating points.

## 2. THEORETICAL ANALYSIS OF THE PHASE SENSITIVITY

To analyze the phase sensitivity of the full and truncated SU(1,1) interferometers, it is useful to consider the phase-sensing potential of the quantum state separately from the phase sensitivity of the entire device, which depends on the chosen detection scheme [17–20]. The phase-sensing potential of the quantum state is identical for both the full and truncated SU(1,1) interferometers, and is related to the quantum Fisher information ${\mathcal{F}}_{Q}$ according to $\mathrm{\Delta}\varphi =1/\sqrt{{\mathcal{F}}_{Q}}$, where ${\mathcal{F}}_{Q}$ is a function of both the two-mode quantum state at the output of the nonlinear medium in Fig. 1 and the particular mode(s) in which the phase object(s) are placed [21]. The phase sensitivity of the measurement is related to the classical Fisher information ${\mathcal{F}}_{C}\le {\mathcal{F}}_{Q}$, where $\mathrm{\Delta}\varphi \ge 1/\sqrt{{\mathcal{F}}_{C}}$ describes the phase sensitivity of the entire device [21]. To optimize the phase-sensing ability of a device, one should choose a measurement scheme such that ${\mathcal{F}}_{C}$ is as close as possible to ${\mathcal{F}}_{Q}$ [20].

Given a measured observable $X$, the phase sensitivity of a measurement device $\mathrm{\Delta}\varphi $ can be evaluated from the signal-to-noise ratio (SNR),

For the present purposes, we make the simplifying assumption that the two modes have identical losses (see Ref. [23] for a more complete model) and that the seed photon number ${|\alpha |}^{2}\gg 1$. The sensitivity depends on the operating point set by the local oscillator phases. Specializing to the case where ${\varphi}_{c}=\pi /2$ (the phase quadrature), but allowing ${\varphi}_{p}$ to vary, one can use the formalism in Ref. [13] and show from Eq. (1) with $\mathrm{SNR}=1$ that the variance of the phase estimation for the truncated SU(1,1) interferometer is

Figure 2 shows the variance of the phase estimation ${\mathrm{\Delta}}^{2}\varphi $ in the case of no loss as a function of the gain of the nonlinear process that produces the two-mode squeezed state. The variance shown in Fig. 2 is defined for the best operating point, e.g., curve (v) is for ${\varphi}_{p}=\pi /2$ in Eq. (3). We also show the variance in phase estimation for the full SU(1,1) interferometer when detecting just the conjugate (unseeded) mode using homodyne detection (scheme ii) or direct intensity detection (scheme iii), as well as direct detection in both modes (scheme iv). (See Supplement 1 for more detailed calculations of the sensitivity for these alternative detection schemes.) Balanced homodyne detection of the joint quadratures substantially improves the phase sensitivity in the seeded truncated and full SU(1,1) interferometers.

In addition, Fig. 2 shows the fundamental bound on the phase sensitivity of the two-mode quantum state used here, as calculated from the quantum Fisher information ${\mathcal{F}}_{Q}$. For the seeded two-mode squeezed state and phase object placement considered here (see Fig. 1) [20],

We note that if the phase object were placed in the lower-power, vacuum-seeded arm, ${\mathcal{F}}_{Q}$ is smaller [20]. The result in Eq. (4) also requires that the measurement has an external phase reference, as shown in Fig. 1, so that the measured sensitivity is independent of the phase of the input beam [21]. One can see in Fig. 2 that ${\mathrm{\Delta}}^{2}{\varphi}_{\mathrm{tSUI}}$ asymptotically approaches the $1/{\mathcal{F}}_{Q}$ bound, and that even at low gain ($G\gtrsim 2$), ${\mathrm{\Delta}}^{2}{\varphi}_{\mathrm{tSUI}}\approx 1/{\mathcal{F}}_{Q}$. The phase-sensing ability of the truncated SU(1,1) interferometer is thus not only equivalent to that of the full SU(1,1) interferometer, but is an optimal measurement choice for sufficiently high gain. For very low gains ($G\lesssim 2$), one can still reach the bound set by the quantum Fisher information using the truncated SU(1,1) interferometer by varying the classical gain of one of the homodyne detectors [24].

In a practical device the losses play an important role and cause the minimum detectable phase shift to increase. In the full SU(1,1) interferometer the internal losses between the nonlinear interactions have a more detrimental effect on the sensitivity than external losses after the second nonlinear interaction [14]. In the truncated SU(1,1) interferometer, all losses are effectively internal losses. While the truncated SU(1,1) interferometer avoids additional internal loss arising from coupling the beams into a second nonlinear device, the full SU(1,1) interferometer has an advantage of being less sensitive to detector losses (see Supplement 1).

In the particular case of Gaussian quantum states and homodyne measurements, the classical Fisher information ${\mathcal{F}}_{C}$ is related to the measurement observable $X$ by [20]

The first term is the inverse of the sensitivity limit determined from the SNR in Eq. (1). If the second term is nonzero, one can achieve a better phase sensitivity by using the change in the distribution as a function of phase [25]. In our scheme, the most sensitive operating point corresponds to the minimum of the joint phase quadrature, at which point ${\partial}_{\varphi}\mathrm{\Delta}X=0$.

## 3. EXPERIMENTAL DEMONSTRATION OF THE TRUNCATED SU(1,1) INTERFEROMETER

We construct the truncated SU(1,1) interferometer using 4WM in a ${}^{85}\mathrm{Rb}$ vapor cell, as depicted in Figs. 3(a) and 3(b) [23]. The nonlinear interaction among the applied beams and the atoms results in an amplified probe and the creation of a correlated conjugate field, where the probe and conjugate fields constitute a two-mode squeezed state. After the cell, the probe and conjugate fields are sent to separate balanced homodyne detectors, as shown in Fig. 3(c).

To detect a specific quadrature, we use piezo-mounted mirrors in the path of each local oscillator to control the phases of each homodyne setup, ${\varphi}_{p}$ and ${\varphi}_{c}$. The AC components ($\approx 1\text{\hspace{0.17em}}\mathrm{MHz}$) of the two homodyne detectors are summed and sent to a spectrum analyzer. The DC components are used to lock the phase of each homodyne detector.

By locking the homodyne detectors to the DC component of the signal, we effectively lock the homodyne detectors to the input phase of the seed beam, indicated by the phase reference line in Fig. 1. This allows us to assess the potential phase-sensing ability of the device without having to build a fully phase-stable interferometer. Likewise, by measuring noise at a convenient high frequency $\mathrm{\Omega}=1\text{\hspace{0.17em}}\mathrm{MHz}$, we avoid technical noise sources. In the absence of technical noise, the noise floor at 1 MHz would extend to DC. The optimal phase sensing is achieved when both homodyne detectors are locked to the phase quadrature of their input beam. This occurs where ${\varphi}_{p}$ and ${\varphi}_{c}$ are locked so that the individual DC homodyne signals are zero and the slopes are the same (see Supplement 1).

An electro-optic phase modulator (EOM) imposes a weak sinusoidal phase shift $\varphi (t)=\sqrt{2}\delta \varphi \text{\hspace{0.17em}}\mathrm{cos}(2\pi \mathrm{\Omega}t)$ on the probe local oscillator, where $\delta \varphi $ is the root mean square amplitude of the phase shift. The signal resulting from this modulation appears on the spectrum analyzer as a peak, shown in Fig. 4(a), with an SNR of ${\mathrm{SNR}}_{\mathrm{tSUI}}$. The signal is generated in the probe detection arm and is determined by $\delta \varphi $ and the probe and local oscillator powers. The noise level is determined by both detection arms, i.e., by the level of squeezing generated by the 4WM process. The reduction in the noise level due to squeezing is the key to achieving quantum-enhanced precision in our system. Both signal and noise vary with the operating point as set by the local oscillator phases. Absent low-frequency technical noise, the modulation frequency could be lowered while keeping a constant SNR. Thus we use this AC signal to infer a sensitivity to DC phase shifts for comparison to the theory given above.

For comparison to this quantum-enhanced measurement procedure, we follow a similar procedure using coherent fields. We turn off the 4WM process by blocking the pump and increase the intensity of the seed beam to create a coherent state probe beam with the same power as the one generated by the 4WM process, resulting in the dashed curve in Fig. 4(a) with an SNR of ${\mathrm{SNR}}_{\mathrm{coh}}$. In this case, ${\mathrm{SNR}}_{\mathrm{tSUI}}-{\mathrm{SNR}}_{\mathrm{coh}}\approx 4\text{\hspace{0.17em}}\mathrm{dB}$.

A previous demonstration of a full SU(1,1) interferometer [15] uses the detection scheme defined by curve (ii, iii) in Fig. 2, which is not the optimal choice of measurement even in the case of no loss. We note that the conventions used in Ref. [15] imply a 3 dB improvement in SNR even at $G=1$, where there are no quantum enhancements.

To characterize the operation of the truncated SU(1,1) interferometer, we compare the ${\mathrm{SNR}}_{\mathrm{tSUI}}$ for a particular choice of local oscillator phases to the optimal ${\mathrm{SNR}}_{\mathrm{coh}}$ (i.e., the SNR when the local oscillator phases are set to give the largest ${\mathrm{SNR}}_{\mathrm{coh}}$). The phase sensitivities are then related to the SNR improvement ($\mathrm{SNRI}={\mathrm{SNR}}_{\mathrm{tSUI}}-{\mathrm{SNR}}_{\mathrm{coh}}$) by

To measure the SNRI as a function of operating point, we lock ${\varphi}_{c}$ to detect the phase quadrature of the conjugate beam and scan ${\varphi}_{p}$. The resulting variation in SNRI is shown in Fig. 4(b). The peaks at ${\varphi}_{p}=\pm \pi /2$ correspond to the operating points with the maximum signal. At ${\varphi}_{p}=\pi /2$, the joint quadrature noise is at its minimum (maximum squeezing). At ${\varphi}_{p}=-\pi /2$, the joint quadrature noise is at its maximum (maximum antisqueezing). The solid curve is a theoretical fit of Eq. (3) to the data with best-fit parameters $\eta =0.65$ and intrinsic gain $G=3.3$. The experimentally measured gain is 2.7, which includes some loss in the vapor cell. For simplicity, we take both arms to have identical loss parameters $\eta $.

The classical Fisher information for this detection scheme in the presence of loss is shown by the dashed line in Fig. 4(b), which is calculated from Eq. (5) using the fit parameters defined above and ${\mathrm{SNRI}}_{{\mathcal{F}}_{C}}=-10\text{\hspace{0.17em}}{\mathrm{log}}_{10}[(1/{\mathcal{F}}_{C})/{\mathrm{\Delta}}^{2}{\varphi}_{\mathrm{coh}}]$. The close overlap of this curve with that derived from ${\mathrm{\Delta}}^{2}{\varphi}_{\mathrm{tSUI}}$ implies that the second term in Eq. (5) is negligible compared to the first.

The standard quantum limit, $\mathrm{\Delta}{\varphi}_{\mathrm{SQL}}$, is usually taken to mean the best sensitivity of a Mach–Zehnder interferometer with intensity detection at both output ports. We compare the truncated SU(1,1) interferometer to a truncated version of a Mach–Zehnder interferometer in which the second beam splitter is replaced with homodyne detectors. The measured signal $X$ is taken to be the difference in the quadrature signals from the two homodyne detectors. At its optimum operating point, this configuration has the same sensitivity as the standard Mach–Zehnder. The SQL depends on the mean number of photons used in the measurement. In the seeded SU(1,1) interferometer, the two beams have different photon numbers, ${N}_{p}$ and ${N}_{c}$ (with ${N}_{c}<{N}_{p}$). Taking the number of photons going through the phase object as the essential resource, we select as the SQL the sensitivity of an ideal Mach–Zehnder with ${N}_{p}=\eta G{|\alpha |}^{2}$ photons detected in the phase-sensing arm, i.e., ${\mathrm{\Delta}}^{2}{\varphi}_{\mathrm{SQL}}=1/(2{N}_{p})$.

To compare our results to the SQL, we need to compare the measured ${\mathrm{SNR}}_{\mathrm{coh}}={(\delta \varphi )}^{2}{N}_{p}$ to that expected for the truncated Mach–Zehnder. We determine ${N}_{p}$ in terms of the probe power and estimated losses, and we find that the measured ${\mathrm{SNR}}_{\mathrm{coh}}$ agrees with the expected value (see Supplement 1). Thus we can conclude that the SNRI measured here shows that the truncated SU(1,1) interferometer achieves a 4 dB improvement in ${\mathrm{\Delta}}^{2}\varphi $ over the SQL, including losses. Further, if we could eliminate all detection losses for the coherent state measurement (see Supplement 1), then ${\mathrm{\Delta}}^{2}{\varphi}_{\mathrm{tSUI}}$, which includes losses, surpasses that by 3 dB. Finally, in the ideal limit of no losses, where the phase sensitivity corresponds to curve (v) in Fig. 2, the SNRI for a gain of 3.3 would be approximately 10.5 dB. The measured value of 4 dB is lower than the ideal value due to losses in the system.

## 4. CONCLUSIONS

We have constructed a novel variation on the SU(1,1) interferometer that removes one nonlinear interaction, and we have measured the SNR of this device as a function of operating point. This arrangement provides a simpler means to achieve quantum-enhanced phase sensitivities, and even with $\approx 35\%$ loss we have demonstrated up to 4 dB improvement over the comparable classical device.

## Funding

National Science Foundation (NSF); Air Force Office of Scientific Research (AFOSR).

## Acknowledgment

We gratefully acknowledge discussions with P. Barberis-Blostein, D. Fahey, and E. Goldschmidt.

See Supplement 1 for supporting content.

## REFERENCES

**1. **V. Giovannetti, S. Lloyd, and L. Maccone, “Advances in quantum metrology,” Nat. Photonics **5**, 222–229 (2011). [CrossRef]

**2. **A. Crespi, M. Lobino, J. C. F. Matthews, A. Politi, C. R. Neal, R. Ramponi, R. Osellame, and J. L. O’Brien, “Measuring protein concentration with entangled photons,” Appl. Phys. Lett. **100**, 233704 (2012). [CrossRef]

**3. **C. M. Caves, “Quantum-mechanical noise in an interferometer,” Phys. Rev. D **23**, 1693–1708 (1981). [CrossRef]

**4. **D. Leibfried, B. DeMarco, V. Meyer, M. Rowe, A. Ben-Kish, J. Britton, W. M. Itano, B. Jelenković, C. Langer, T. Rosenband, and D. J. Wineland, “Trapped-ion quantum simulator: experimental application to nonlinear interferometers,” Phys. Rev. Lett. **89**, 247901 (2002). [CrossRef]

**5. **C. Gross, T. Zibold, E. Nicklas, J. Estève, and M. K. Oberthaler, “Nonlinear atom interferometer surpasses classical precision limit,” Nature **464**, 1165–1169 (2010). [CrossRef]

**6. **M. Xiao, L.-A. Wu, and H. J. Kimble, “Precision measurement beyond the shot-noise limit,” Phys. Rev. Lett. **59**, 278–281 (1987). [CrossRef]

**7. **P. Grangier, R. E. Slusher, B. Yurke, and A. LaPorta, “Squeezed-light—enhanced polarization interferometer,” Phys. Rev. Lett. **59**, 2153–2156 (1987). [CrossRef]

**8. **H. Yonezawa, D. Nakane, T. A. Wheatley, K. Iwasawa, S. Takeda, H. Arao, K. Ohki, K. Tsumura, D. W. Berry, T. C. Ralph, H. M. Wiseman, E. H. Huntington, and A. Furusawa, “Quantum-enhanced optical-phase tracking,” Science **337**, 1514–1517 (2012). [CrossRef]

**9. **M. J. Holland and K. Burnett, “Interferometric detection of optical phase shifts at the Heisenberg limit,” Phys. Rev. Lett. **71**, 1355–1358 (1993). [CrossRef]

**10. **G. Y. Xiang, B. L. Higgins, D. W. Berry, H. M. Wiseman, and G. J. Pryde, “Entanglement-enhanced measurement of a completely unknown optical phase,” Nat. Photonics **5**, 43–47 (2010). [CrossRef]

**11. **M. W. Mitchell, J. S. Lundeen, and A. M. Steinberg, “Super-resolving phase measurements with a multiphoton entangled state,” Nature **429**, 161–164 (2004). [CrossRef]

**12. **B. Yurke, S. L. McCall, and J. R. Klauder, “SU(2) and SU(1, 1) interferometers,” Phys. Rev. A **33**, 4033–4054 (1986). [CrossRef]

**13. **W. N. Plick, J. P. Dowling, and G. S. Agarwal, “Coherent-light-boosted, sub-shot noise, quantum interferometry,” New J. Phys. **12**, 083014 (2010). [CrossRef]

**14. **A. M. Marino, N. V. Corzo Trejo, and P. D. Lett, “Effect of losses on the performance of an SU(1, 1) interferometer,” Phys. Rev. A **86**, 023844 (2012). [CrossRef]

**15. **F. Hudelist, J. Kong, C. Liu, J. Jing, Z. Y. Ou, and W. Zhang, “Quantum metrology with parametric amplifier-based photon correlation interferometers,” Nat. Commun. **5**, 3049 (2014). [CrossRef]

**16. **Z. Y. Ou, “Enhancement of the phase-measurement sensitivity beyond the standard quantum limit by a nonlinear interferometer,” Phys. Rev. A **85**, 023815 (2012). [CrossRef]

**17. **U. Dorner, R. Demkowicz-Dobrzanski, B. J. Smith, J. S. Lundeen, W. Wasilewski, K. Banaszek, and I. A. Walmsley, “Optimal quantum phase estimation,” Phys. Rev. Lett. **102**, 040403 (2009). [CrossRef]

**18. **J. Kong, Z. Y. Ou, and W. Zhang, “Phase-measurement sensitivity beyond the standard quantum limit in an interferometer consisting of a parametric amplifier and a beam splitter,” Phys. Rev. A **87**, 023825 (2013). [CrossRef]

**19. **D. Li, C.-H. Yuan, Z. Y. Ou, and W. Zhang, “The phase sensitivity of an SU(1, 1) interferometer with coherent and squeezed-vacuum light,” New J. Phys. **16**, 073020 (2014). [CrossRef]

**20. **C. Sparaciari, S. Olivares, and M. G. A. Paris, “Gaussian-state interferometry with passive and active elements,” Phys. Rev. A **93**, 023810 (2016). [CrossRef]

**21. **M. Jarzyna and R. Demkowicz-Dobrzański, “Quantum interferometry with and without an external phase reference,” Phys. Rev. A **85**, 011801 (2012). [CrossRef]

**22. **H. Bachor and T. Ralph, *A Guide to Experiments in Quantum Optics* (Wiley, 2004).

**23. **C. F. McCormick, A. M. Marino, V. Boyer, and P. D. Lett, “Strong low-frequency quantum correlations from a four-wave-mixing amplifier,” Phys. Rev. A **78**, 043816 (2008). [CrossRef]

**24. **B. E. Anderson, B. L. Schmittberger, P. Gupta, K. M. Jones, and P. D. Lett, “Optimal phase measurements with bright and vacuum-seeded SU(1,1) interferometers,” arXiv:1704.04261 (2017), accepted for publication in Phys. Rev. A.

**25. **L. Pezzé, A. Smerzi, G. Khoury, J. F. Hodelin, and D. Bouwmeester, “Phase detection at the quantum limit with multiphoton Mach–Zehnder interferometry,” Phys. Rev. Lett. **99**, 223602 (2007). [CrossRef]