Using states with a large photon number variance to increase quantum Fisher information in single-mode phase estimation

TL;DR

This paper identifies specific quantum states with large photon number variance that can enhance phase estimation precision in quantum metrology, encouraging experimental exploration of these states.

Contribution

It introduces particular states with high photon number variance that could improve quantum Fisher information in phase estimation.

Findings

Identified states with large photon number variance.

These states can potentially improve local phase estimation.

Encourages experimental realization of the proposed states.

Abstract

When estimating the phase of a single mode, the quantum Fisher information for a pure probe state is proportional to the photon number variance of the probe state. In this work, we point out particular states that offer photon number distributions exhibiting a large variance, which would help to improve the local estimation precision. These theoretical examples are expected to stimulate the community to put more attention to those states that we found, and to work towards their experimental realization and usage in quantum metrology.

Equations

$$|{\psi }_{\text{SSW}}⟩$$

$$|{\psi }_{\text{SS}}⟩$$

$$|{\psi }_{\text{Dowling}}⟩$$

$$|{\psi }_{\text{SMP}}⟩$$

$$\Delta \varphi \ge \frac{1}{\sqrt{\nu H}},$$

$$H=4⟨(\Delta \hat{n}{)}^2⟩$$

$$H_{\text{sq}}=8(N^2+N),$$

$$|{\psi }_{\text{b}}⟩=\sum _{n=m}^M\sqrt{p(n)}{e}^{i\theta (n)}|n⟩,$$

$$⟨(\Delta \hat{n}{)}^2⟩\le \frac{1}{4}(M-m{)}^2,$$

$$⟨(\Delta \hat{n}{)}^2⟩\le (M-N)(N-m),$$

$$|{\psi }_{\text{m\&M}}⟩=\sqrt{1-a}|m⟩+\sqrt{a}|M⟩.$$

$$H_{\text{m\&M}}=4a(1-a)(M-m{)}^2.$$

$$|{\psi }_{\text{m\&M}}⟩=\sqrt{\frac{M-N}{M-m}}|m⟩+\sqrt{\frac{N-m}{M-m}}|M⟩,$$

$$H_{\text{m\&M}}=4(M-N)(N-m).$$

$$p_{\text{G}}(n)=\mu (1-\mu {)}^n,$$

$$⟨(\Delta \hat{n}{)}^2{⟩}_{\text{G}}=N^2+N.$$

$$p_{\text{NB}}(n)=\left(\genfrac{}{}{0ex}{}{n+\eta -1}{n}\right){\mu }^n(1-\mu {)}^{\eta }$$

$$⟨(\Delta \hat{n}{)}^2{⟩}_{\text{NB}}=N^2+\frac{\mu \eta (1-\mu \eta )}{(1-\mu {)}^2}.$$

$$p_{\text{L}}(n)=\{\begin{array}{ll}0& \text{for }n=0,\\ \frac{-1}{\ln (1-\mu )}\frac{{\mu }^n}{n}& \text{for }n\ge 1,\end{array}$$

$$⟨(\Delta \hat{n}{)}^2{⟩}_{\text{L}}=N^2+\frac{-\mu [2\mu +\ln (1-\mu )]}{(1-\mu {)}^2[\ln (1-\mu ){]}^2}.$$

$$p_{\text{B}}(n)=\{\begin{array}{ll}0& \text{for }n=0,\\ \frac{e^{-\mu n}(\mu n{)}^{n-1}}{n!}& \text{for }n\ge 1,\end{array}$$

$$⟨(\Delta \hat{n}{)}^2{⟩}_{\text{B}}=\mu /(1-\mu {)}^3=N^2(N-1),$$

Full text

I Introduction

Finding an optimal combination of an input state and a measurement setup is one of the key issues in quantum metrology, by which quantum enhancement can be maximized Giovannetti et al. (2011). On the one hand, the optimality of a measurement setting is assessed by comparing the Fisher information for a chosen setting with the quantum Fisher information (QFI) that would be obtained by an optimal setting, given parameter encoding and a probe state Paris (2009); Oh et al. (2019). The optimality of a probe state, on the other hand, can be addressed by maximizing the QFI given a parameter encoding Dorner et al. (2009). The aforementioned approaches apply to various parameter estimation problems.

Much attention has been paid on identifying optimal quantum states in a variety of quantum metrological applications. The attention has been triggered because the key mechanism leading to quantum enhancement can often be understood as the non-classicality of the probe state Giovannetti et al. (2006, 2011); Kwon et al. (2019). For example, in single-mode loss parameter estimation, the photon number state having no uncertainty in the intensity is known to be the optimal state, providing the maximal quantum enhancement Adesso et al. (2009); Nair (2018). In phase parameter estimation, it is known that the squeezed vacuum state reaches the QFI scaled with $N^{2}$ Monras (2006), leading to a Heisenberg scaling of $N^{-1}$ in precision, where $N$ is the average photon number of the probe state. However, the squeezed vacuum state is not the theoretical optimal state that maximizes the QFI in single-mode phase estimation as we will discuss through this work.

Various fiducial photon number distributions have so far been considered as candidates to achieve quantum enhancement in single-mode phase estimation. Examples include the SSW state Shapiro et al. (1989), the SS state Shapiro and Shepard (1991), Dowling’s model Dowling (1991), the small peak model Braunstein (1994); Rivas and Luis (2012). These states are respectively written in the photon number state basis $\{\left|{n}\right\rangle\}$ by

[TABLE]

where the ${\cal N}$’s correspond to normalization factors, $z$ is a positive constant, $\eta$ is a smooth cutoff, $0\leq a\leq 1$, and $\left|{\pi}\right\rangle$ is orthogonal to the vacuum. Different approaches have been employed to show the advantages of such states in phase estimation.

In this work, we begin with the appreciation that the QFI for the single-mode phase parameter estimation is proportional to the photon number variance of the probe state and sets the lower bound in the precision through the quantum Cramér-Rao inequality Braunstein and Caves (1994); Braunstein et al. . This implies that the probe state with the maximal photon number variance would possibly be the theoretical optimal state for single-mode phase estimation. Here, we aim to introduce, while leaving the proof of the achievability of the quantum Cramér-Rao bound to future studies Rubio et al. (2018); Rubio and Dunningham , fiducial quantum states that have the maximum, or at least a larger photon number variance than that available with the squeezed vacuum state – the paradigmatic state known to be useful for quantum phase estimation. We distinguish the scenarios when the photon number probability distribution is either bounded or unbounded, i.e., defined within a finite or an infinite domain James (2006). When considering bounded distributions, we show that the theoretical optimal state with maximum photon number variance can indefinitely increase the QFI even for a fixed average photon number $N$. When considering unbounded distributions, we show that one can achieve not only the Heisenberg scaling using other quantum states than the squeezed vacuum state, but also sub-Heisenberg scaling by a particular photon number statistics without relying on any nonlinear effects. Here, the sub-Heisenberg scaling manifests in terms of the average photon number $N$ and might mislead to conclude that it violates the fundamental Heisenberg limit. More details on that can be found in the relevant debates, which have been devoted over the last decade Bollinger et al. (1996); Yurke et al. (1986); Sanders and Milburn (1995); Ou (1996); Zwierz et al. (2010); Luis and Rodil (2013); Luis (2013); Anisimov et al. (2010), followed by the conclusive proofs Zwierz et al. (2010); Tsang (2012); Giovannetti and Maccone (2012); Giovannetti et al. (2012); Berry et al. (2012); Hall et al. (2012); Hall and Wiseman (2012a, b); Jarzyna and Demkowicz-Dobrzański (2015). The latter showed that the overall scaling, while including the amount of resources required for obtaining a priori probability distribution of the parameter and the number of measurements required to achieve the asymptotic bound, is still Heisenberg scaling-limited. Nevertheless, the fiducial photon number distributions we introduce here would be useful for an operating regime of a parameter that is locally calibrated in advance, so the identification of minute changes of the parameter is only of interest. That is, fortunately, often the case, e.g., for plasmonic sensors Lee et al. (2017, 2018) or phase tracking Yonezawa et al. (2012). In such cases, the validity of the quantum Cramér-Rao bound can be investigated in terms of the required minimum number of measurements and the minimum prior knowledge of the parameter Rubio et al. (2018); Rubio and Dunningham .

The theoretical states we discuss in this work have rarely been experimentally realized so far McCormick et al. (2019), but we expect more states will be implemented in the future. It would require the development of quantum technology geared towards engineering states with photon number statistics on demand. Recently, an arbitrary photon number statistics has been shown to be producible with current technology through quantum optical circuits being optimized for a target photon number statistics F. Dell’Anno and Illuminati (2006); Bimbard et al. (2010); Nichols et al. ; Arrazola et al. (2019). Having the ability to prepare such quantum states unlocks their use for various purposes in quantum applications O’Driscoll et al. (2019). Therefore, the purpose of this work is to lay out exotic photon number distributions in order to trigger experimental efforts along these lines.

II Phase estimation

For a parameter-encoded pure state $\left|{\psi_{\phi}}\right\rangle=e^{i\phi\hat{G}}\left|{\psi_{\text{in}}}\right\rangle$, where $\hat{G}$ denotes a generator encoding a parameter $\phi$, the QFI can be calculated by $H=4\langle(\Delta\hat{G})^{2}\rangle$ Braunstein and Caves (1994); Braunstein et al. , where $\langle(\Delta\hat{O})^{2}\rangle=\langle\hat{O}^{2}\rangle-\langle\hat{O}\rangle^{2}$ for an operator $\hat{O}$ and the expectation value is calculated for $\left|{\psi_{\text{in}}}\right\rangle$. The QFI sets the lower bound to the mean-squared-error of estimate when considering an unbiased estimator, given by the quantum Cramér-Rao inequality written as

[TABLE]

where $\Delta\phi$ is the root-mean-squared-error, interpreted as the estimation error or precision, and $\nu$ denotes the number of repetitions of measurement. This bound, called quantum Cramér-Rao bound, is known to be achievable in the asymptotic limit $\nu\rightarrow\infty$.

For a single-mode phase parameter encoding, $\hat{G}=\hat{a}^{\dagger}\hat{a}$, so that the QFI is given by

[TABLE]

where $\hat{n}=\hat{a}^{\dagger}\hat{a}$. This clearly indicates that a probe state $\left|{\psi_{\text{in}}}\right\rangle$ with a maximum photon number variance leads to the maximal QFI. The importance of the photon number fluctuation for phase estimation has been addressed Hofmann (2009); Hyllus et al. (2010). In consequence, the maximum photon number variance leads to the greatest quantum enhancement over the standard quantum limit (SQL), i.e., $\Delta\phi$ scaled with $N^{-1/2}$ Leonhardt et al. (1995). Such scaling is the optimal scaling that can be obtained when only classical resources are used Pirandola et al. (2018). Therefore, it is of utmost importance to identify quantum states with a maximum photon number variance.

To set the stage before looking for particular photon number distributions, let us consider a few of paradigmatic states that have often been considered for phase estimation. The first one is a coherent state $\left|{\alpha}\right\rangle$ of light, for which $H_{\text{coh}}=4N$, where the average photon number is $N=\left|\alpha\right|^{2}$ Monras (2006). $H_{\text{coh}}$ is regarded as the classical benchmark in single-mode phase estimation, i.e., the SQL. Another example is a squeezed vacuum state written as $\left|{\xi}\right\rangle=\sum_{n}c_{n}\left|{2n}\right\rangle$ where $c_{n}=(-e^{i\theta_{\text{s}}}\tanh r)^{n}\sqrt{(2n)!}/\left(2^{n}n!\sqrt{\cosh r}\right)$ with the squeezing parameters $r$ and $\theta_{\text{s}}$. For the squeezed vacuum state, the QFI reads as Monras (2006)

[TABLE]

where the average photon number is given as $N=\sinh^{2}r$. It is clear that $H_{\text{sq}}$ exhibits a Heisenberg scaling, which suggests that $\Delta\phi$ scales with $N^{-1}$ [see Eq. (5)]. In particular, one can see that $H_{\text{sq}}\approx 504.89$ for state-of-the-art squeezed state of 15 dB-squeezing as recently reported Vahlbruch et al. (2016), approximately corresponding to $r\approx 1.73$ (i.e., $N\approx 7.46$) while ignoring the thermal photon contribution for simplicity despite its practical significance studied in Refs. Aspachs et al. (2009); Šafránek and Fuentes (2016); Oh et al. (2019, ).

In the next sections, we look for quantum states with maximum photon number variance, or at least larger than that of the squeezed vacuum state, which consequently further increases the QFI in Eq. (6) as compared to $H_{\text{sq}}$ of Eq. (7). To this end, we distinguish two types of discrete probability distributions $p(n)$ for photon number statistics of a single-mode probe state: a bounded photon number distribution that is defined within a finite domain $n\in[m,M]$ with integers $m<M$ and an unbounded photon number distribution that is defined in an infinite domain $n\in[0,\infty)$.

III Bounded photon number distributions

For the sake of generality, let us consider an arbitrary superposition of photon number states in a range from $m$ to $M$ photons, written as

[TABLE]

where the photon number distribution $p(n)$ is bounded by the minimum $m$ and the maximum $M$, i.e., $p(n)=0$ for $n<m$ and $n>M$. The phase distribution $\theta(n)$ plays an important role in preparing an optimal measurement setting in practice, which depends on both $\theta(n)$ and $\phi$ being estimated. The phases, however, can be dismissed in this work since we focus on the error bound given by the QFI. This means that the optimal measurement setting assumed to be chosen accommodates the phases, leaving only the dependence of $p(n)$ in Eq. (6). One can find that the variance of such bounded probability distribution $p(n)$ is upper bounded by Popoviciu’s inequality Popoviciu (1935), given as

[TABLE]

where the equality holds when $p(m)=p(M)=1/2$. This implies that for the given minimum $m$ and maximum $M$, a balanced superposition of $m$ and $M$ photons provides the maximal QFI according to Eq. (6). The QFI is thus written as $H=4(M-N)^{2}$ with $N=(m+M)/2$ being the average photon number. For a fixed $N$, the maximal QFI is obtained when $m=0$, which is obvious, for which $H=4N^{2}$, clearly showing the Heisenberg scaling, but still smaller than $H_{\text{sq}}$ in Eq. (7). The bound on $\Delta\phi$ associated Popoviciu’s inequality indicates that the Heisenberg scaling is the maximal scaling when the photon number distribution is bounded.

A stronger inequality than Eq. (9) exists, called the Bhatia–Davis inequality Bhatia and Davis (2000), which is written as

[TABLE]

where the equality holds when $p(n)=1-a$ and $p(M)=a$ for an arbitrary weight factor of $a$ that determines the average photon number $N=(1-a)m+aM$. When $a=1/2$, the Bhatia-Davis inequality of Eq. (10) becomes the Popoviciu inequality of Eq. (9). The Bhatia-Davis inequality suggests to consider an arbitrary superposition state of $m$ and $M$ photons, which we call the m&M state throughout this work. The m&M state can be written as

[TABLE]

This leads to the QFI of the form

[TABLE]

It is clear that $H_{\text{m\&M}}$ depends on the difference $(M-m)$ and takes on the maximum when $a=1/2$ for given $m$ and $M$, the case satisfying the equality of Popoviciu’s inequality. To compare the QFIs for a fixed $N$, let us set $a=(N-m)/(M-m)$ which keeps $N$ unchanged for any $m$ and $M$, so that Eq. (11) is rewritten by

[TABLE]

and Eq. (12) becomes

[TABLE]

Note that $N$ is fixed in Eq. (14) regardless of the values of $m$ and $M$ although Eq. (14) seems directly obtainable from Eq. (10) where $N$ definitely depends on $m$ and $M$. It is interesting to see that in the limit $M\gg N$, one obtains $H_{\text{m\&M}}\approx 4M(N-m)$, which can be arbitrarily increased by increasing $M$ while keeping $N$ fixed.

Equation (14) indicates that the QFI increases with increasing the maximum $M$ and decreasing the minimum $m$ for a fixed $N$. So let us set $m=0$, for which the m&M state of Eq. (13) becomes the 0&M state, i.e., $\left|{\psi_{\text{0\&M}}}\right\rangle=\sqrt{(M-N)/M}\left|{0}\right\rangle+\sqrt{N/M}\left|{M}\right\rangle$, for which $H_{\text{0\&M}}=4N(M-N)$. Therefore, the 0&M state is the optimal state and $H_{\text{0\&M}}$ is the upper bound for the QFI within the class of the states having a bounded photon number distribution. The 0&M state has been considered as the so-called ON states in the context of quantum computation Sabapathy and Weedbrook (2018) and a few schemes for its experimental generation have been proposed Yukawa et al. (2013); Arrazola et al. (2019). The 0&M state has already been discussed as the state showing an arbitrarily large QFI in single-mode phase estimation Berry et al. (2012); Luis (2017), but here we prove, by using the Bhatia-Davis inequality of Eq. (10), that the 0&M state is the theoretical optimal state exhibiting the maximum photon number variance among the states with bounded photon number distributions.

The 0&M state can be categorized as the small peak model of Eq. (4). In general, the QFI for the small peak model is given as $H_{\text{SMP}}=4N(N_{\pi}-N)+4(\Delta n_{\pi})^{2}N/N_{\pi}$, where $N_{\pi}$ is the average photon number of the state $\left|{\pi}\right\rangle$ and $(\Delta n_{\pi})^{2}$ denotes its variance. The small peak model is able to attain an arbitrarily large QFI by increasing either $N_{\pi}$ or $(\Delta n_{\pi})^{2}$, while keeping $N$ fixed. The particular case $\left|{\pi}\right\rangle=\left|{\xi}\right\rangle$ has been discussed in Ref. Rivas and Luis (2012), followed by the review in Ref. Berry et al. (2012).

In comparison with Eq. (7), for $N=7.46$ considered in state-of-the-art squeezed vacuum state, one can achieve higher QFI than $H_{\text{sq}}$ with the 0&M state when $M\geq 25$ (corresponding to $a\lesssim 0.3$), resulting in $H_{\text{0\&M}}\gtrsim 523.39$. Figure 1 shows the behaviors of $H_{\text{0\&M}}$ (see red curve) and $a=N/M$ (see dashed curve) with varying $M$ for $N=7.46$. Note that $H_{\text{0\&M}}$ in the order of $10^{5}$ can be theoretically attained by increasing $M$ even when $N$ is fixed. The 0&M state has been realized up to $M=18$ in the harmonic motion of a single trapped ion McCormick et al. (2019), and the states with higher $M$ can also be realized in quantum optical circuits with current technology Nichols et al. ; Arrazola et al. (2019); O’Driscoll et al. (2019).

IV Unbounded photon number distributions

When a probability distribution is defined in an infinite domain, i.e., unbounded, there exits an infinite number of degrees of freedom to characterize types of unbounded probability distribution. Therefore, the analysis for unbounded photon number distributions would not be as simple as the bounded case. Instead, we investigate here a few special probability distributions, which lead to intriguing behaviors in single-mode phase estimation.

IV.1 Heisenberg scaling in the local precision

As mentioned above, the squeezed vacuum state enables the Heisenberg scaling of $N^{-1}$ in $\Delta\phi$. It is interesting to see that there exist other types of photon number statistics, leading to the Heisenberg scaling in phase estimation. Below, let us look at some of them as examples.

Consider the probe state with the photon number distribution given as

[TABLE]

for $\mu\in(0,1)$. This is called the geometric distribution and $p_{\text{G}}(n)$ is the probability of $n+1$ Bernoulli trials required to get the first success with success probability $\mu$. It possesses the average photon number of $N=(1-\mu)/\mu$ and the variance of

[TABLE]

This clearly exhibits the Heisenberg scaling through Eq. (6), i.e., scaling of $N^{-1}$ in $\Delta\phi$, although a little worse than the case using a squeezed vacuum state due to the absence of the factor of 2.

A generalization of the geometric distribution, called the negative binomial distribution, can also be considered, written by

[TABLE]

for $\mu\in(0,1)$ and $\eta>0$. In this case, the average photon number is given by $N=\mu\eta/(1-\mu)$ while the variance takes the form of

[TABLE]

Note that the second term is positive only when $\mu\eta<1$, for which the Heisenberg scaling is achieved. When $\mu\eta>1$, on the other hand, a worse scaling than the Heisenberg scaling is obtained. It can be shown that the states with $p_{\text{NB}}(n)$ significantly outperforms the case using a squeezed vacuum state when $\mu\eta<1$ and $\mu\approx 1$.

As another example, consider the probe state with the photon number distribution given as

[TABLE]

for $\mu\in(0,1)$. This is called the logarithmic distribution and has been used to model relative species abundance Johnson et al. (2005). It exhibits the average photon number of ${N=-\mu/(1-\mu)\ln(1-\mu)}$ and the variance of

[TABLE]

Here, the second term plays an important role in determining a further improvement when compared to the case using a squeezed vacuum state. The second term is negative when $\mu<\mu_{\text{c}}$. It crosses zero to be positive at $\mu=\mu_{\text{c}}$, and increases to diverge when increasing $\mu$ further, where $\mu_{c}\approx 0.7968$ is the solution of $2\mu+\ln[1-\mu]=0$. One can see that the corresponding QFI is less than $H_{\text{sq}}$ for $\mu\ll 1$ (i.e., $N\ll 1$), but outperforms $H_{\text{sq}}$ when $\mu\approx 1$ (i.e., $N\gg 1$).

IV.2 Sub-Heisenberg scaling in the local precision

The Heisenberg scaling of $N^{-1}$ in $\Delta\phi$ is considered as the ultimate scaling in quantum parameter estimation, often called the Heisenberg limit. It has been shown that a sub-Heisenberg scaling 111In the literature, the terms “super-Heisenberg scaling” and “sub-Heisenberg scaling” have interchangeably used to denote the same limit Boixo et al. (2008); Woolley et al. (2008); Rams et al. (2018); Roy (2019). of $N^{-s}$ with $s>1$ is achievable through nonlinear effects arising in many-body systems Boixo et al. (2007, 2008); Choi and Sundaram (2008); Roy and Braunstein (2008); Woolley et al. (2008); Napolitano and Mitchell (2010); Rams et al. (2018). The latter has been demonstrated with a nonlinear atomic ensemble Napolitano et al. (2011). Here we show that a similar sub-Heisenberg scaling can also be achieved by particular photon number statistics of a single-mode state of light, but requiring neither nonlinearity nor many-body systems. Note that such alluring results do not indicate that the Heisenberg limit can be beaten, but have been proved to be still limited by the Heisenberg scaling when appropriately accounting of all the resources needed to reach the error bound Zwierz et al. (2010); Tsang (2012); Giovannetti and Maccone (2012); Giovannetti et al. (2012); Berry et al. (2012); Hall et al. (2012); Hall and Wiseman (2012a, b); Jarzyna and Demkowicz-Dobrzański (2015).

Consider the state with the photon number distribution given by

[TABLE]

for $\mu\in[0,1]$. The distribution $p_{\text{B}}(n)$ is called Borel distribution Borel (1942); Tanner (1961), being observed in branching process and queueing theory Otter (1949); Haight and Breuer (1960). The distribution of Eq. (21) exhibits the average photon number of $N=1/(1-\mu)$ and the variance of

[TABLE]

obviously leading to the QFI of $H_{\text{B}}=4N^{2}(N-1)$. Therefore, the probe state engineered with photon number distribution of $p_{\text{B}}(n)$ promises sub-Heisenberg scaling of $N^{-3/2}$ in $\Delta\phi$, being dominant in the limit $N\gg 1$, i.e., when $\mu\approx 1$. Again, note that it has been proven that sub-Heisenberg strategies are not so effective Giovannetti and Maccone (2012), but would provide rather insignificant improvement when taking into account a priori knowledge about the parameter $\phi$.

IV.3 Indefinite scaling in the local precision

Unlike the bounded probability distribution, there is no upper bound to the variance of the unbounded probability distribution. In other words, some probability distribution may have a diverging or even an infinite variance, arising from the feature of heavier tails than the exponential distribution Foss et al. (2013). One can consider distributions such as the Riemann-Zeta distribution, the Beta negative binomial, or the Yule-Simon distribution, all of which exhibit a diverging or an infinite variance of the photon number. Particularly, the Riemann Zeta distribution has already been considered as an interesting example showing an infinite QFI in two-mode schemes Zhang et al. (2013). These examples seem to provide the completely precise estimation, but it turned out that it is not the case (see more detailed discussion in Ref. Berry et al. (2012)).

V Conclusion

We have identified particular fiducial photon number distributions of a single-mode probe state, which maximize the QFI and would possibly be useful for the local phase estimation. Considering the case that the photon number distribution is bounded, we have provided the proof that the theoretical optimal state is the 0&M state, indefinitely increasing the QFI and consequently reducing the local estimation error of $\Delta\phi$ in the asymptotic limit of the number of measurements $\nu\rightarrow\infty$. For the case that the photon number distribution is unbounded, on the other hand, we have discussed several particular photon number statistics which show Heisenberg scaling and sub-Heisenberg scaling without requiring nonlinear effects. The states discussed in this work have rarely been experimentally realized McCormick et al. (2019), but state-of-the-art quantum state engineering technique would enable the generation of an arbitrary photon number superposition via quantum circuit optimization Nichols et al. ; Arrazola et al. (2019); O’Driscoll et al. (2019). In the scenario when a priori probability distribution of the parameter is unknown and the number of measurements is limited, those states may not be useful since they are still Heisenberg-scaling limited with $N_{\text{tot}}=N\nu$, the total average number of photons being used. It has been shown that the strong Heisenberg limit written as $\Delta\phi_{\text{s}}\propto 1/N_{\text{tot}}$ Pezzè and Smerzi (2008); Giovannetti et al. (2004, 2011); Tsang (2012); Giovannetti et al. (2012); Berry et al. (2012); Hall et al. (2012); Giovannetti and Maccone (2012); Hall and Wiseman (2012b, a) can never be beaten Shapiro et al. (1989); Shapiro and Shepard (1991); Hradil and Shapiro (1992); Hradil (1992); Braunstein et al. (1992); Braunstein (1992); Lane et al. (1993); Braunstein (1994); Anisimov et al. (2010); Rivas and Luis (2012); Luis and Rodil (2013); Luis (2013); Zhang et al. (2013); Demkowicz-Dobrzański et al. (2012); Pezzé (2013). However, when estimating the parameter in a local regime, the states we discussed would be able to provide the sub-Heisenberg scaling in principle. Furthermore, Luis recently showed through analytical and numerical examination that the weak Heisenberg limit Pezzé et al. (2015), written as $\Delta\phi_{\text{w}}\propto 1/\sqrt{\nu}N$, can be beaten by the 0&M state with the prior information being updated without bias Luis (2017).

More rigorous analysis beyond the framework of the quantum Cramér-Rao bound is necessary to see whether or not the states discussed in this work can beat at least the weak Heisenberg limit for practical purposes Rubio et al. (2018); Rubio and Dunningham . We leave similar investigation for unbounded photon number distributions as a future study. From a more fundamental perspective, the relation between the QFI and quantum coherence can be investigated for the states discussed in this work Streltsov et al. (2017); Giorda and Allegra (2018); Tan et al. (2018); Kwon et al. (2018). From a practical perspective, on the other hand, the effect of loss or decoherence needs to be taken into account when the local precision is more rigorously examined. These subtle analyses are beyond the scope of this work, and so we leave them for future work. It would also be interesting to investigate other kinds of single-mode parameter estimation or multi-mode schemes. Particularly, in the Mach-Zehnder interferometer, useful states within the class of path-symmetric states have been discussed in terms of the QFI in Ref. Lee et al. (2016). One can generalize it to an arbitrary two-mode setting for full generality.

acknowledgments

We acknowledge support by the KIT-Publication Fund of the Karlsruhe Institute of Technology. S.-Y. Lee was supported by a grant to Quantum Frequency Conversion Project funded by Defense Acquisition Program Administration and Agency for Defense Development. C. Oh and H. Jeong were supported by the National Research Foundation of Korea (NRF) through grants funded by the Ministry of Science and ICT (Grant Nos. 2019R1H1A3079890 and NRF-2019M3E4A1080074 ).