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Showing posts with label nationalism. Show all posts
Taiwanese nationalism is not your grandfather's nationalism
The other day a classmate on my graduate program, after asking me about Taiwan and hearing my response that the opinion of a strong majority of Taiwanese leans towards considering Taiwan already independent, or at least certainly not Chinese, referred to the idea of 'nationalism' with a strongly negative connotation. He wasn't necessarily critiquing Taiwan specifically, but rather the general idea that a group wanting to form their own nation is a concept riddled with problems.
He was surprised when I replied that Taiwanese nationalism is not ethnic nationalism, and the two can't be conflated in such a reductionist way.
I certainly understood what he meant - he even brought up the old-timey concept of 'nationalism' that arose in Europe in the late 19th and early 20th centuries, where every 'group' or ethnicity has their own little country and therefore what it means to be a country is based primarily on ethnic ties, leaving aside of course the idea that ethnicity itself is an odd and problematic construct. Basically, that often "nationalism" is considered to be inextricably linked with ethnocentrism.
I, too, have an instinctive reaction against this worldview because this view of nation-hood (and what it means to be a nation, and who should be within the borders of one or a citizen of one) are so deeply linked to my family history. The Armenians and other non-Turks were massacred not primarily because of religion (although it played a part), but because the old construct of the Ottoman Empire as a multi-ethnic, multi-territorial "empire" was washed away by the Young Turks in favor of what was then a more "modern" view of nationhood, where one nation ought to equal one ethnicity. The Armenians were not Turks, and therefore, according to this view, they had to go.
Over a million Armenians died, and I exist as a result of this sort of ethnocentric nationalism sweeping Turkey in 1915. Although I am happy I exist - not that I would know if I didn't - I am all too aware of how far off the rails this idea can go.
China takes this a step further and promotes an unrealistic view of what it means to be 'Chinese', trying to force not just the same national identity but also the same ethnic identity on, essentially, whomever it wishes. It also tries to discredit Taiwan's case for de jure nationhood by playing to liberal perceptions of the problems of nationalism. It's no accident that they call Taiwanese nationalism 'splittism' and try to tap into the negative connotations associated with, say, voting for Brexit, ethnic regions splitting off from a larger nation and civil war. China also tries to promote the positive connotations that we associate with being stronger or 'better together' than apart. China tries to have it both ways - any desire to not be a part of China is 'splittism', and Xinjiang and Tibet are a part of China despite their people not being 'Chinese', however, Taiwan is a part of China because 'we're the same'. So people who are not Chinese are Chinese because China controls them and that's okay, but China should control Taiwan specifically because Taiwanese are, they say, Chinese and not some other kind of people.
If that's not clear or seems like it doesn't make sense, that's because it isn't and doesn't. Nothing about China's argument makes a lick of sense, in fact, but it seems to have been accepted by huge swaths of the educated world.
(Side note: although I don't generally believe in ethnic nationalism, I don't necessarily always think it's wrong for an ethnic group to want to break off a piece of territory to form its own nation, especially if mistreatment of that group is involved. Each situation is highly unique, and I can't really say one blanket solution is applicable, not being intimately familiar with the various examples of this).
So why is the lumping of Taiwanese nationalism in with the sort of nationalism popular in our grandparents' generation so inaccurate?
Simple - it's not based on ethnicity. Not really, anyway.
Some Taiwan independence activists do try to make an ethnicity-based argument for their cause, pointing, for example, to evidence that Taiwan is primarily ethnically Austronesian rather than Chinese (note: the writer of that post doesn't necessarily agree - I don't know and it doesn't matter - but the post itself is pertinent).
I think most, though, know that this is a losing proposition. Not because they're necessarily wrong about who the Taiwanese are at the DNA level, but because even if they convince the world that Taiwan is "not Chinese", they'll face the argument that ethnic nationalism has its own problems and therefore isn't necessarily something to support. It opens up a messy argument on what it means to be "ethnically Taiwanese", which opens us up to having to defend that position.
And, frankly, they know it wouldn't matter: China didn't take ethnicity into account when taking over Tibet and Xinjiang. If not the same old "we are all Chinese" blather, they'll find another argument because their goal, to them, will always justify the means by which they attain it.
It just doesn't matter much and won't work.
In any case, who are the Taiwanese? DNA testing shows a large correlation with Austronesian/SE Asian populations. But what about those who aren't - whose grandparents really did come from China and whose families haven't intermarried much with locals? Are they not Taiwanese? How about those who might have Japanese blood, or one non-Taiwanese parent? How about those who were born and raised here, whose parents aren't Taiwanese at all? If you make this argument, you leave all of them out, not to mention those of us who would like dual nationality, all to argue a point that China doesn't actually care about, and will hurt Taiwan's case to the world rather than help it, by making Taiwan independence seem like another iteration of 'ethnic nationalism'.
So if Taiwanese nationalism is not that - and I don't think it is - what is it?
You could say it's a nationalism based on Taiwan's unique history, and there is truth to that, but I don't know about you, but I'm not interested in getting into a pointless history debate with an anti-Taiwan detractor and I don't think it's a very strong argument either. Although history is on our side, who owned what in the past just isn't the way to make the case for Taiwan. It actually weakens what I think is the best argument, in fact.
Instead, Taiwanese nationalism is based on the idea that Taiwan is a nation based on two things: self-determination and shared values.
It is hard to imagine a reasonable person disagreeing with the idea that people have the right to self-determination, although we can reasonably disagree with the level at which that right manifests itself (e.g. that the citizens of a nation have that right, but that a group wishing to secede their territory from that nation may perhaps not always have it). I'd say there's a case to be made that any self-ruled territory that has an independently functioning government gains that right, and Taiwan certainly falls well within that boundary. It's even a democracy so you can't argue that a territory has been wrested away by some strongman dictator!
Therefore, as a self-governing autonomous territory that has a highly functional and democratic government, Taiwan does have the right to determine its own future. Period. This would be true even if history weren't on our side.
As for shared values, this is trickier. As much as different segments of Taiwanese society might disagree on a variety of issues, pretty much all of them except for a few ancient blowhards can agree on a few basic principles: human rights including certain freedoms, democracy and egalitarianism (okay, maybe not everyone agrees with egalitarianism in practice, but that's a global problem). However you define "shared values", though, it's clear that the values that are important in Taiwanese society are vastly different from those allowed in Chinese society. They also differ to some extent from the values even of other Asian democracies, despite greater similarities with those nations.
The good news is that this means Taiwanese nationalism doesn't suffer from having a weak or outdated argument. We're not 'splittists', 'separatists' (wanting to separate from what? When was Taiwan ever a part of the People's Republic of China that we'd be wanting to now 'split off'?) or people causing 'ethnic tensions'. Taiwan is instead a sovereign state that simply wants to access a right to globally recognized self-determination, and build their democratic nation based on shared values.
We have an optics problem, not an argument problem. There is nothing wrong with our case. I would like to think that optics problems are easier to solve.
Basically, this updated, 21st century view of nationalism - as nation-building based on shared values and the right to self-determination rather than ethnicity - is much easier for the global literati to swallow. It's an argument that humanizes Taiwan, and presents it in a modern light appropriate to its situation and values, rather than making it sound like an outdated and even dangerous throwback to the ethnocentrism and 'small European nation state' model of a few generations ago. It sounds more like something an EU supporter would say, and less like something a nutbar UKIP or Trump voter would come out with.
It's just as good news that this weakens China's "argument", such as it is. When you view Taiwanese as not ethnic nationalists, which they are indeed not in any great majority, China's case that Taiwan is a part of China because 'we are all Chinese' makes even less sense, and forces them to defend ethnic nationalism. Better yet, it forces them to defend it alongside claiming territories like Xinjiang and Tibet despite not having this connection.
It's also good news in that this view of nationalism allows - and please allow me to be selfish here - for people like me to be a part of these shared values. I can never be, and don't want to be, 'Asian' or 'Chinese' simply because I think it's weird to want to change one's race (and creepy and appropriative for a white person in any case). However, viewing Taiwan as a nation of people of shared values rather than a nation of people who were born ethnically Taiwanese with no 'outsiders' allowed makes room for people like me. Under such a model, I could be Taiwanese. Under an ethnic model, I could not.
The bad news is that many supporters of Taiwan don't seem to have made this connection. I don't mean that they don't support foreigners naturalizing (though some don't), but that they just don't think it's a big issue or something that needs to be prioritized or even necessarily changed. Some, perhaps, have not quite come to the conclusion that if Taiwan is not a country based on ethnicity but one of shared values and self-determination, that that means you kinda sorta have to let in immigrants because if you don't, you're right back at ethnic nationalism and all the problems it entails.
The other bad news is that China's been bombarding the world with a skewed perspective on what Taiwanese nationalism is, promoting whatever definition of 'nationalism' is convenient to them, and it's very hard to re-orient the perspectives of those who've bought that particular brand of snake oil.
All I can say is that we need to keep trying, and we absolutely need to stop engaging China on the points it's tempting us with, e.g. trying to argue ethnicity or history. Even if we're right - and we are - we absolutely need to not only re-shape the internal debate of Taiwanese nationalism being one of values rather than blood, which many astute friends of Taiwan are already doing, but also to point out to the international community that Taiwanese nationalism does not share the deeply problematic worldview and chauvinism of our grandparents' ethnic nationalism.
Labels: being_taiwanese, dual_nationality, international_discourse, nationalism, politics, taiwanese_history, taiwanese_independence, thoughts


Online High School Credits offers a rating system from one to five stars for online high school programs. We put our heads together and decided on some important points that we would look for if we were going to enroll a student into a quality online program. Some of these school systems range from free to several thousand dollars a year. You have lots of online school systems out there to choose from and we hope to make it easier on you to make a educated decision from the beginning.
(0.5 / 5) We award an extra .5 star if the online high school is accredited by more than one agency or group making for a total of 1.5 stars.
(0.5 / 5) We add .5 star if the school also provides a guidance counselor or advisor along with the student's teachers.
(0.5 / 5) We award .5 stars for flexibility of schedule and accessibility of classes.
(1 / 5) We award 1 star if the program offers good electives, AP-College Prep, or Dual Enrollment courses.
(0.5 / 5) If the school has a good website that is informative and easy to use, we award .5 stars.
If a school has all of these requirements, they can get a total of 5 stars (5 / 5), but if they have a website with information that is not easily available and/or clear, we may award that school zero stars based solely on that availability, even though they still may be an excellent school.
**NOTE TO SCHOOLS: If you have a school listed on this list and the school has zero stars because we simply cannot access the information from your website, you are welcome to contact us with information in order for us to change your star rating.


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\section{Introduction}
In the optical domain, the high density of optical states implies that the interaction between a single optical mode and an emitter is usually weak. As a consequence, single-photon sources, nonlinear photon-photon interactions, and photonic quantum gates are inefficient. These limitations can be overcome by placing single quantum emitters in photonic nanostructures where the routing of photons into a guided mode can be highly efficient. Additionally the interaction between a single photon and a single quantum emitter needs to be coherent, which entails that a distinct phase relation is maintained when a single photon is scattered from the emitter, i.e., incoherent broadening mechanisms must be efficiently suppressed. Such a lifetime-limited photon-emitter interface enables indistinguishable single-photon sources~\cite{Santori2002,He2013,Ding2016,Senellart2017,Kirsanske2017}, quantum optical nonlinearities at the single photon level~\cite{Javadi2015,Maser2016,Snijders2016,DeSantis2017,Hallett2017,Chang2014} and may find applications in quantum many-body physics~\cite{Suter2016}. Consequently, many different solid-state quantum platforms are currently under development, each of which is based on a specific quantum emitter~\cite{Birnbaum2006,Sipahigil2016,Maser2016,Bhaskar2017,Javadi2017,Turschmann2017} and with its own strengths and weaknesses. A coherent and deterministic photon-emitter interface may be a building block for complex architectures in quantum communication, towards the ultimate goal of distributed photonic quantum networks~\cite{Kimble2008,Ritter2012,Lodahl2017}.

Epitaxially grown quantum dots (QDs) embedded in GaAs membranes are the basis for a particularly mature platform, as they are now routinely integrated into a variety of nanophotonic structures~\cite{Lodahl2015}. By molding the photonic environment of QDs at their native nanoscale the emitted single photons can be coupled to a guided mode with near-unity efficiency~\cite{Arcari2014} and made highly indistinguishable~\cite{Ding2016,Kirsanske2017}. The access to lifetime-limited resonance linewidths is a stricter requirement than that of indistinguishability of subsequently emitted photons since the former requires suppression of both slow drift (charge or spin noise)~\cite{Kuhlmann2013} and fast pure dephasing (phonon decoherence)~\cite{Thoma2016,Tighineanu2016}. Remarkably, this can be obtained by embedding QDs in electrically-contacted bulk semiconductor structures~\cite{Kuhlmann2015}. However, exposed etched surfaces present in nanophotonic structures may pose a problem since they could induce charge noise in the samples.  Here, we address this issue and demonstrate near lifetime-limited photon-QD interaction in a nanophotonic waveguide. This is an essential step towards a deterministic on-chip few-photon nonlinearity, which could form the basis of, e.g., a deterministic Bell-state analyzer~\cite{Ralph2015} and is a prerequisite for coupling multiple QDs.

\begin{figure}[tb]
\begin{center}
\includegraphics[width=0.95\columnwidth]{fig1_ver7.pdf}
  \caption{Resonant transmission spectroscopy on a QD in a nanobeam waveguide. (a) Sketch of the sample, which includes a QD embedded in a nanobeam waveguide that is terminated with a circular grating out-coupler. For the RF (RT) measurements the QD is excited from free-space (the waveguide thought the circular grating input-coupler), respectively; in both cases, the output signal is top-collected from the grating. (b) Calculated electric field profile of the primary mode of the nanobeam waveguide. (c) Illustration of a QD ideally coupled to the waveguide (green box), in which case all on-resonance (orange) photons are reflected while off-resonance (red) photons are transmitted, as described by a Lorentzian lineshape with a width limited by the lifetime of the QD (green curve). Adding pure dephasing (blue) effectively leads to a smearing out of the excited state, thereby lowering the efficiency of the light-matter interaction and resulting in the partial transmission of on-resonant photons and a broadening of the transmission dip (blue curve). Reducing the emitter-waveguide coupling efficiency reduces the depth of the dip in both cases.}
\label{fig:f1_system}
\end{center}
\end{figure}

Figure~\ref{fig:f1_system}(a) shows the layout of the experiment. Two types of coherent measurements are performed on a QD that is efficiently coupled to a waveguide: resonant fluorescence (RF) and resonant transmission (RT) measurements. In RF, the QD is excited at the emitter's resonance frequency $\omega_0$ from free-space and subsequently emits photons into the guided mode with a probability determined by the $\beta$-factor. The photons are subsequently coupled out of the waveguide at a distant location with a circular grating and detected.

In RT, the QD is excited through the waveguide by a weak laser and the interference between the scattered and incident photons is recorded. RT measurements on a QD were first reported in Ref.~\citenum{Hogele2004}. For a QD ideally coupled to the waveguide ($\beta = 1$) and in the absence of dephasing ($\Gamma_d = 0$), the scattered and incident light interferes destructively and incident single photons resonant with the QD transition are reflected, as sketched in Figure~\ref{fig:f1_system}(c). When detuned off-resonance, the photons do not interact with the QD and are consequently transmitted. A finite pure dephasing rate $\Gamma_d$ effectively smears out the energy levels and partially destroys the quantum coherence between the scattered and transmitted photons. This allows on-resonance photons to be transmitted and broadens the QD resonance, cf. illustration in Figure~\ref{fig:f1_system}(c).

The resonant scattering leads to a Lorentzian extinction dip in the transmission spectrum, whose depth depends on the effective emitter-waveguide coupling efficiency $\beta$ and the pure dephasing rate of the emitter $\Gamma_d$. Here $\beta \neq 1$ is due to the photons that are not scattered into the waveguide mode, including the fraction of photons that are emitted into the phonon sideband~\cite{Besombes2001,Favero2003}. The power dependent transmission intensity on resonance is given by \cite{Javadi2015}
\begin{equation}\label{eq:T}
    T= 1+ \frac{(\beta-2)\beta}{(1+2\gamma_\mathrm{r})(1+S)},
\end{equation}
where $\gamma_\mathrm{r} =\Gamma_d/\Gamma$ is the pure dephasing rate relative to the homogeneous linewidth $\Gamma$ and $S=n_\tau/n_c$ quantifies the effective saturation of the QD transition. $n_\tau$ is the mean photon number of photons within the lifetime of the emitter input field that is normalized by a critical input flux
\begin{equation}\label{eq:nc}
 	n_c = \frac{1+2\gamma_{\mathrm{r}}}{4\beta^2},
\end{equation}
which represents the number of photons in the waveguide within the lifetime of the emitter resulting in an excited state population of 1/4 for the QD. The corresponding width of the Lorentzian trough is given by
\begin{equation} \label{eq:linewidth}
\Gamma_\mathrm{RT} = (\Gamma + 2 \Gamma_d)\sqrt{1+S}.
\end{equation}
We note that a larger dephasing rate $\Gamma_d$ causes the extinction dip to both widen and lessen, as resonant photons that would otherwise be reflected are transmitted instead. In contrast, a non-ideal coupling $(\beta<1)$ only reduces the depth for a fixed decay rate. It is therefore possible to extract both $\beta$ and $\Gamma_d$ in the weak excitation limit $(n_\tau \ll n_c)$ from Eq.~\eqref{eq:T} if the homogeneous linewidth $\Gamma$ is known independently from lifetime measurements. The $\beta^2$ dependence of $T$ in Eq.~\eqref{eq:T} makes the minimum transmission a sensitive probe of the effective $\beta$-factor whereas the dephasing rate $\Gamma_d$ can be extracted from the measured linewidth. At larger incident powers the QD transition is power broadened, as seen from Eq.~\eqref{eq:linewidth}, and results in a decrease of the transmission extinction.

In the following experiment the waveguide sample featured weak reflections from the termination ends, meaning that weak cavity resonances were modulating the spectral response of the system. Consequently, the transmission response has a Fano spectral character~\cite{Shen2005,Auffeves-Garnier2007,Javadi2015}, which slightly modifies the Lorentzian profile that Eq. (\ref{eq:linewidth}) describes. See Supplementary Information for detailed expressions for the Fano resonances that were used to model the experimental data.

The experiment is conducted on a single QD located near the center of a \SI{600}{\nano\meter} wide and \SI{175}{\nano\meter} thick planar GaAs nanobeam waveguide. The width was chosen to maintain a relatively large separation between the QD and nearby interfaces while still supporting a well-confined mode (see Figure~\ref{fig:f1_system}(b)) with a large $\beta$-factor above 0.5. The waveguide supports three guided modes and the higher order modes can largely be filtered out via photonic elements on the chip (see Supplementary Information). The studied QD is located approximately \SI{15}{\micro\meter} away from the collection grating, which is a second-order circular Bragg grating optimized for a wavelength of \SI{920}{\nano\meter}~\cite{Faraon2008}, cf. Figure \ref{fig:f1_system}(a) with a full SEM image of the sample shown in Supplementary Information. The QD layer with a density of around $\SI{1}{\micro\meter}^{-2}$ is embedded in a p-i-n diode (see Ref.~\citenum{Kirsanske2017} for details) and held at a temperature of \SI{1.7}{\kelvin} in order to stabilize the local charge environment and to suppress phonon broadening~\cite{Besombes2001,Favero2003,Tighineanu2016}. Charge stabilization is essential in order to achieve narrow optical linewidths~\cite{Lobl2017}. We consider a bright neutral exciton line $X^0$ of the QD with an emission wavelength of \SI{920.86}{\nano\meter} at \SI{0.2}{\volt}, cf. Figure~\ref{fig:f2_RFnRT}(a) with other charge states being visible at longer wavelengths. The external bias enables tuning of the QD transition energy. The decay rate of the QD is measured by time correlated single photon counting on an avalanche photo diode (APD) with a response time of \SI{50}{\pico\second} where the QD is excited by a picosecond-pulsed laser tuned to the p-shell at \SI{905.8}{\nano\meter}. Excitation in the p-shell prevents the excitation of free carriers, which could shield the QD from the applied field and thus potentially modify the decay rate. The measured decay curve is shown in the inset in Figure~\ref{fig:f2_RFnRT} and is fitted with a single exponential decay convoluted with the measured instrument response function (IRF) of the APD. The extracted decay rate is $\gamma = \SI{5.49\pm 0.02}{\per\nano\second}$ corresponding to a natural linewidth of $\Gamma =\gamma/2\pi =\SI{0.87\pm 0.003}{\giga\hertz}$ and a lifetime of $\tau = 1/\gamma = \SI{182}{\pico\second}$. For comparison the decay rate recorded on QDs in an unstructured part of the sample is around $\gamma = \SI{3.5}{\per\nano\second}$. This corresponds to a Purcell factor of 1.6 in the nanobeam waveguide, which is consistent with simulations for a QD located within \SI{20}{\nano\meter} from the waveguide center (see Supplementary Information).

The large decay rate (short lifetime) of the QDs found both in bulk and in nano structures for the present wafer is attributed to a large QD oscillator strength \cite{Lodahl2015}. To exclude non-radiative processes, a lower estimate of the internal quantum efficiency of the QDs was determined from measurements on two QDs on the same chip embedded in photonic-crystal waveguides, where the coupling to the waveguide strongly modifies the radiative decay rate. Here we observed an inhibited decay rate of $\gamma_i = \SI{1.2}{\per\nano\second}$ for a QD spectrally located inside the photonic band gap region. For comparison a greatly enhanced decay rate of up to $\gamma_e = \SI{13.5}{\per\nano\second}$ was observed for a QD coupled to the photonic crystal waveguide. A lower-bound estimate assumes that the inhibited rate $\gamma_i$ is dominated by non-radiative processes and we can extract an internal quantum efficiency of $\eta_{QE} \geq (\gamma_e-\gamma_i)/\gamma_e \approx{92} \%$, i.e., it can be excluded that the short lifetimes originate from non-radiative recombination.

\begin{figure}[tb]
\begin{center}
\includegraphics[width=0.8\columnwidth]{fig_RF_RT_lw_spectrum.pdf}
\caption{Photoluminescence spectroscopy on a single QD. (a) Voltage dependent photoluminescence map (bottom panel) of the QD under above-band excitation. Full spectrum of the QD recorded at $V=\SI{0.2}{\volt}$ is shown in the top panel. Linewidth measurement from the resonance fluorescence (b) and the resonant transmission (c) configuration for the $X^0$ QD transition.The solid red curves represent a Lorentzian fit to the data and the Fano resonance model (cf. Supplementary Information for the detailed expression), respectively. A nearby residual peak from the same QD is modelled with a Lorentzian function as well, and excluded from the analysis. Inset in (b): Measured decay curve of the QD. The red line is the fit to a single-exponential model. The measurements were done at a sample temperature of $T=\SI{1.7}{\kelvin}$.}
\label{fig:f2_RFnRT}
\end{center}
\end{figure}

The RF spectrum is presented in Figure~\ref{fig:f2_RFnRT}(b), which was measured by scanning the frequency of a narrow-band continuously-tunable diode laser (Toptical CTL with $<\SI{10}{\kilo\hertz}$ bandwidth) from the top across the QD resonance at a fixed bias voltage of $V=\SI{0.2}{\volt}$. The incident laser and collection are co-polarized transversely to the waveguide mode where the spatial separation between the QD and the collection grating is sufficient to achieve an RF signal that is more than 200 times larger than the background laser. The lineshape is well modelled by a Lorentzian with a linewidth of $\Gamma_\mathrm{RF} = \SI{1.12 \pm 0.03}{\giga\hertz}$. The RF experiment was conducted at an excitation intensity of $S=0.13$ of the saturation level, meaning that power broadening amounts to a linewidth increase of 6\%. The Lorentzian lineshape is evidence that the additional broadening is dominated by pure dephasing, and we estimate a pure dephasing rate of $\Gamma_d = \num{0.14}\Gamma$. The observed nearly transform-limited linewidth shows that electrical gating of planar nanophotonic structures may overcome residual broadening due to charge noise~\cite{Liu2017}.

For the RT measurements the laser is injected into the waveguide through an input circular grating coupler (see Supplementary Information for an electron microscope image) and then mode filtered through a photonic crystal waveguide followed by a single mode section to predominantly inject light into one waveguide mode. The RT spectrum on the same QD at a low excitation power of $S=0.02$ is presented in Figure~\ref{fig:f2_RFnRT}(c). Here the laser frequency is fixed at $\omega/2\pi = \SI{325.457}{\tera\hertz}$ while the QD transition frequency $\omega_0/2\pi$ is tuned by the voltage over the p-i-n diode. A coarse frequency-voltage scan is used to calibrate the local frequency axis. We observe a narrow extinction of the resonant transmission with a linewidth of $\Gamma_\mathrm{RT} = \SI{0.96 \pm 0.07}{\giga\hertz}$, which is only broadened by 10 \% relative to the natural linewidth. The near transform-limited linewidth implies that a record-high extinction of $\Delta T =  0.66\pm 0.04$ is obtained, which is more than 1.5 times larger than previously reported for solid-state emitters integrated into nanophotonic waveguides~\cite{Javadi2015,Bhaskar2017,Turschmann2017,Hallett2017}. The extinction quantifies the strength of coherent interaction between a single photon and the QD and is therefore an essential figure-of-merit for quantum-information processing \cite{Lodahl2015}.

The transmission spectrum in Figure~\ref{fig:f2_RFnRT}(c) is modelled with the full spectral model\cite{Javadi2015} that accounts for the effective $\beta$-factor, pure dephasing $\Gamma_d$, and coupling to Fabry-–P\'erot modes in the waveguide arising from residual reflections from the termination of the waveguide structure. This coupling leads to an extra phase shift and results in the asymmetric Fano-like lineshape observed in Figure~\ref{fig:f2_RFnRT}(c). We extract $\beta = \num{0.51 \pm 0.04}$ and a pure dephasing rate of $\Gamma_d = (\num{0.06 \pm 0.04})\Gamma$, i.e. the transmission response is nearly transform limited.  For comparison the calculated pure dephasing rate is $\Gamma_d \approx \num{0.01}\Gamma$ based on the contributions from phonons\cite{Tighineanu2016}, which is consistent with the experimental results.
We note that the \SI{600}{\nano\meter} wide nanobeam supports three guided modes at the operation wavelength of \SI{920}{\nano\meter}, and the extracted $\beta$ is therefore to be considered an effective coupling efficiency, i.e. the coupling to the dominating mode can be even higher.

\begin{figure}[tb]
\begin{center}
\includegraphics[width=0.98\columnwidth]{fig_trans_vs_power_1010.pdf}
 \caption{Saturation behavior of the resonant transmission. The transmission dip (a) and the QD linewidth (b) as a function of power at $T=\SI{1.7}{\kelvin}$. The transition linewidth broadens and the transmission extinction decreases as the emission intensity of the neutral exciton transition saturates at a characteristic input power of \SI{13.1}{\nano\watt} corresponding to that on average $\sim 1.6$ photons interact with the QD within its radiative lifetime. When the emitter is saturated, the transmission is dominated by the resonant laser and reaches the steady value of one. The homogeneous linewidth $\Gamma = \SI{0.87}{\giga\hertz}$ is shown as a dashed green line. The red lines are consistent model fits to the purple data points while the blue data points are omitted in the fit since the extracted values are influenced by the neighboring transition that is apparent in the data of Figure~\ref{fig:f2_RFnRT} and that influences the analysis at elevated pump power.}
\label{fig:f3_PowerSeries}
\end{center}
\end{figure}

The analysis reveals that the linewidth recorded from the RF data ($\Gamma_\mathrm{RF} = \SI{1.12 \pm 0.03}{\giga\hertz}$) is slightly larger than the value obtained from the RT measurement ($\Gamma_\mathrm{RT} = \SI{0.96 \pm 0.07}{\giga\hertz}$). The two experiments are conducted with different experimental conditions: in the former case \SI{15.7}{\nano\watt} (corresponding to 13.5 photons/lifetime) of laser power is directed to the waveguide while in the latter only \SI{26}{\pico\watt} of optical power travels through the waveguide (see Supplementary Information for the detailed description). It is therefore plausible that the higher excitation intensity applied in the RF experiment may introduce a slight inhomogeneous broadening, e.g., due to light-induced activation of charge defect states introducing spectral diffusion~\cite{Kuhlmann2015,Kurzmann2016}. Excitingly such broadening seems to be absent in the RT experiment, where the only remaining decoherence mechanism is pure dephasing, which broadens the zero-phonon line and can potentially be suppressed at low temperatures by phonon engineering~\cite{Tighineanu2016}. Note that the phonon sidebands effectively rescale the $\beta$-factor, and may be improved by enhancing the radiative decay rate through, e.g., Purcell enhancement~\cite{Lodahl2015}. Consequently our work shows that the planar nanophotonic platform grants access to all required tools for constructing a fully deterministic and coherent photon-emitter interface $(\beta \simeq 1, \Gamma_d \simeq 0)$ at optical frequencies.

\begin{figure*}[tp]
\begin{center}
\includegraphics[width=0.9\textwidth]{fig_RT_temp.pdf}
\caption{Temperature dependent resonant transmission. (a) Transmission spectra recorded at \SI{0.68}{\nano\watt} and at a temperature varied from 1.97 to \SI{30}{\kelvin} (curves from bottom to top). The shallow dip and  narrow peak observed at the low energy side of the main feature are attributed to the resonance of another transition and another QD, respectively. The QD resonance red shifts with temperature (see the inset), thus the voltage needed to map out the resonance is increased. The red line in the inset is a model fit to the band edge shift (see Supplementary Information). Linewidth and corresponding dephasing rate (b) and minimum (c) of the transmission resonance as a function of temperature. The red line is a guide to the eye, which illustrates the variation of the linewidth. This data set has been taken in a non-ideal polarization, where multiple waveguide modes were collected with a different $\beta$-factor, thus the transmission extinction for low temperature slightly differs slightly from that observed in Figure~\ref{fig:f2_RFnRT} and \ref{fig:f3_PowerSeries}.}
\label{fig:f4_Temperature}
\end{center}
\end{figure*}

In order to show the nonlinear interaction with the QD, power dependent RT measurements were carried out. For each incident power a transmission spectrum similar to Figure \ref{fig:f2_RFnRT}(c) is recorded and the extracted transmission minimum and linewidth are presented in Figure~\ref{fig:f3_PowerSeries}. We note that the neighboring peak in Figure \ref{fig:f2_RFnRT}(b) influences the analysis of the linewidth at higher powers, which induces fluctuations in the data in Figure~\ref{fig:f3_PowerSeries}.
The experimental data are well explained by the theory for power broadening: as the excitation power increases, the coherence of the scattered light is reduced and the transmission converges towards unity (cf. Figure~\ref{fig:f3_PowerSeries}(a)). Correspondingly the linewidth broadens, cf. Figure~\ref{fig:f3_PowerSeries}(b). The description of the modelling of the data is given in the Supplementary Information.
The characteristic input power determining the saturation of the coupled QD corresponds to that on average $\sim 1.6$ photons in the waveguide interact with the QD per emitter lifetime.

Finally, the robustness of the observed behavior to temperature is mapped out in detail. Figure~\ref{fig:f4_Temperature} shows RT measurements at a low power of $P=\SI{0.7}{\nano\watt}$ and as a function of temperature. The spectra are acquired by keeping the resonant laser fixed and scanning the voltages across the p-i-n diode. We find a  nonlinear temperature dependence of the central position of the resonance, see the inset of Figure~\ref{fig:f4_Temperature}(a), which is explained by the temperature dependence of the band edge of the semiconductor material. From the data series we can extract the temperature dependence of the decoherence processes. Figure~\ref{fig:f4_Temperature}(b) shows the recorded temperature dependence of the linewidth and the corresponding pure dephasing rate obtained by modelling the transmission spectra. The temperature dependence of the transmission extinction is shown in Figure~\ref{fig:f4_Temperature}(c). Up to about \SI{10}{\kelvin}, the linewidth remains nearly transform limited and the pure dephasing rate is therefore small.  The linewidth broadens significantly at higher temperatures, which reflects the cross-over between different temperature regimes in the pure dephasing rate, as predicted by theory \cite{Tighineanu2016}.

We have demonstrated that highly efficient and coherent quantum light-matter interaction can be obtained in nanoscale planar waveguides, by using electrically-contacted GaAs nanophotonic structures with embedded InAs QDs. In particular, we present lifetime-limited linewidth measurements of QDs as recorded in a resonance transmission experiment. The coherent and efficient coupling manifests itself in a large scattering extinction at the single-photon level  of up to $\Delta T = 0.66$, which is more than 1.5 times larger than what has been previously reported\cite{Hallett2017}. Future work will focus on increasing the $\beta$-factor even further, which can be straightforwardly done by decreasing the waveguide width in order to be in the single-mode regime while the potential influence of charge noise should still be eliminated. Consequently, a clear path-way to a  high-cooperativity photon-emitter interface is laid out, which may enable photonic quantum gates implemented on a fully solid state platform~\cite{Reiserer2015}. Furthermore, the exploitation of coherent nonlinear quantum optics and collective effects~\cite{Chang2014} provides an interesting future direction.

\begin{acknowledgement}
We gratefully acknowledge financial support from the European Research Council (ERC  Advanced Grant ``SCALE''), Innovation Fund Denmark (Quantum Innovation Center ``Qubiz''), and the Danish Council for Independent Research. R.S., A.D.W. and A.L. acknowledge support within the DFG SFB ICRC - TRR 160 Z1 project and BMBF - Q.com-H 16KIS0109. M.C.L., I.S., and R.J.W. acknowledge financial support from NCCR QSIT and from SNF Project No. $200020\_175748$.
\end{acknowledgement}

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  Ludwig,~A.; Warburton,~R.~J. \emph{Phys. Rev. B} \textbf{2017}, \emph{96},
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  Verma, Mirin, Nam, Song, Ma, Chen, Ni, Niu, and Srinivasan]{Liu2017}
Liu,~J.; Konthasinghe,~K.; Davanco,~M.; Lawall,~J.; Anant,~V.; Verma,~V.;
  Mirin,~R.; Nam,~S.~W.; Song,~J.~D.; Ma,~B.; Chen,~Z.~S.; Ni,~H.~Q.;
  Niu,~Z.~C.; Srinivasan,~K. \textbf{2017}, arXiv:1710.09667\relax
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  Geller]{Kurzmann2016}
Kurzmann,~A.; Ludwig,~A.; Wieck,~A.~D.; Lorke,~A.; Geller,~M. \emph{Appl. Phys.
  Lett.} \textbf{2016}, \emph{108}, 263108\relax
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Reiserer,~A.; Rempe,~G. \emph{Rev. Mod. Phys.} \textbf{2015}, \emph{87},
  1379--1418\relax
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\end{mcitethebibliography}

\clearpage

\section*{Supporting Information}

\renewcommand{\theequation}{S\arabic{equation}}
\renewcommand{\thefigure}{S\arabic{figure}}

\setcounter{figure}{0}
\setcounter{equation}{0}

\section*{Coupling efficiency and emission enhancement}
We investigate a quantum dot (QD) that is embedded in the symmetry plane $y=0$ of a \SI{600}{\nano\meter} wide and 175 nm thick, suspended GaAs $n=3.6)$ nanobeam waveguide. Such a waveguide supports three guided optical modes, which we calculate using a finite-element eigenmode
solver (COMSOL Multiphysics) and show in Figure~\ref{fig:App_Modes}.
\begin{figure}
\begin{centering}
\includegraphics[width=13cm]{Modes_fig}
\par\end{centering}
\caption{Three guided modes supported by a \SI{600x180}{\nano\meter} suspended GaAs nanobeam waveguide, all of which are clearly confined to the high index region. The fundamental (TE0) and second-order mode (TE2) posses an even symmetry with respect to the center of the waveguide ($x=0$ axis), while the first-order mode (TE1) is evenly symmetric and has zero amplitude at the center. \label{fig:App_Modes}}
\end{figure}
Here, the amplitude of the dominant (transverse, $E_{x}$) field component is shown, and the mode order can be determined by the number of nodes that it contains. For all three modes, TE0-TE2, the peak amplitude is found on the $y=0$ symmetry plane of the waveguide, which is where the QDs are located. Only the TE0 and TE2 modes have non-zero transverse electric field amplitude at the center of the waveguide $x=0$, meaning that only these modes will couple to a QD located near $x=0,y=0$.

The coupling of the QDs to the photonic modes is characterized by the $\beta$-factor, which for mode $m$ can be defined as the ratio of the power radiated by the emitter (dipole) into the preferred mode to the total power radiated by the dipole,
\begin{equation}
\beta_{m}=\text{P}_{m}^\mathrm{rad}/\text{P}_\mathrm{tot}^\mathrm{rad}.\label{eq:App_BetaInP}
\end{equation}
It can be extracted from full-vectorial three-dimensional numerical simulations (COMSOL Multiphysics, frequency domain) of the nanobeam waveguide with an embedded dipole, most simply by recalling that the power radiated by a dipole oscillating with a frequency $\omega$
is
\begin{equation}
\text{P}=\frac{\omega}{2}\operatorname{Im}\left(\boldsymbol{d}^{*}\cdot\boldsymbol{E}\right),\label{eq:App_dipolePower}
\end{equation}
where $\boldsymbol{d}$ is the electric dipole moment, which in our
case is $\boldsymbol{d}=d\hat{\boldsymbol{x}}$ (and for convenience
we set $d=1$). That is, determining the power radiated by the dipole
reduces to finding $E_{x}$, and more specifically we can rewrite
Eq.~\eqref{eq:App_BetaInP} as\cite{Rotenberg2017}
\begin{equation}
\beta_{m}=\frac{\operatorname{Im} [E_{m,x}\left(x_{0,}y_{0,}z\rightarrow\infty\right)]}{\operatorname{Im} [E_{x}\left(x_{0,}y_{0,}z_{0}\right)]},\label{eq:App_betaM}
\end{equation}
which holds as long as there is no loss in the waveguide. Here, the dipole is located at $(x_{0},y_{0},z_{0})$ and so the denominator is proportional to the total power radiated by the dipole. Extracting the numerator is slightly more involved, particularly in a multi-mode waveguide. First, we note that one does not need to calculate the field at infinity and it is sufficient to consider the field several $(\approx 5)$ wavelengths (inside the waveguide) away from the dipole position, where the non-guided contribution to the electric field is negligible. We account for the multi-modal nature by Fourier transforming $E_{x}$ extracted from the simulations\cite{Rotenberg2017}, and filtering out one-mode at a time in $k$-space to calculate the coupling efficiency for each mode.

Figure \ref{fig:App_betaAndEta} shows the calculated $\beta_{m}$ for the three guided modes as the emitter is moved away from the center (in $x$).
\begin{figure}
\begin{centering}
\includegraphics[width=11cm]{beta_purcell}
\par\end{centering}
\caption{Coupling efficiency and emission enhancement in our nanobeam waveguide as a function of emitter displacement from the center of the waveguide (in $x$). Top panel: Position dependent $\beta$-factor for the three guided modes, and their sum for an $x$-oriented dipole. These clearly follow the line-shape of $\left|E_{x}\right|,$ as shown in Figure~\ref{fig:App_Modes}, with the coupling to TE0 and TE1 peaking near the center of the waveguide, and the coupling to TE1 increasing as that of TE0 decreases. Note that the total coupling efficiency to the guided modes remains near unity over the whole waveguide. Bottom panel: Total emission enhancement (to all modes) as a function of emitter position. The complex lineshape arises due to the multi-mode nature of the waveguide. \label{fig:App_betaAndEta}}
\end{figure}
Both the coupling to the TE0 and TE1 modes are observed to peak near $x=0$, with values near 0.5. The coupling efficiency to TE0 decreases monotonically as the emitter is displaced from the center, while the coupling to TE2 first decreases then increase again after about 100 nm. That is, the spatial dependency of $\beta$ follows that of $|E_{x}|$ for each mode, as expected from Eq.~\eqref{eq:App_dipolePower}. Likewise, the TE1 mode does not couple to the emitter at the center of the waveguide, but $\beta_{TE1}$ increases to about 0.5 for displacements near \SI{150}{\nano\meter}.

The total emission enhancement due to the presence of the nanobeam waveguide
can also be extracted from our three-dimensional simulations. This
emission enhancement, known as the Purcell factor, is simply the ratio of the power emitted by the dipole
in the nanostructure to that emitted by an identical dipole in a homogeneous
medium,
\begin{equation}
F_{P}=\frac{\operatorname{Im}[E_{x}^\mathrm{nano}\left(x_{0,}y_{0,}z_{0}\right)]}{\operatorname{Im}[E_{x}^\mathrm{hom}\left(x_{0,}y_{0,}z_{0}\right)]},
\end{equation}
where the numerator can be recognized from Eq.~\eqref{eq:App_betaM}, and the denominator is similarly extracted from a numerical simulation of an identical dipole in a homogeneous (GaAs) medium. As shown in the bottom panel of Figure~\ref{fig:App_betaAndEta}, we find $F_{P}=1.65$ at the center of the waveguide, which first decreases to about 1.4 for a displacement of \SI{75}{nm} and then increase to about 1.75 near \SI{175}{\nano\meter}. The complex line shape of $F_{P}$ arises because, at different positions, the dipole interacts differently with the different modes.

\section*{Device}
An electron-microscope image of the entire nanophotonic device is shown in Figure \ref{fig:App_SEM}. The light is coupled via the rightmost grating, after which it propagates through a photonic crystal waveguide, which filters out the TE1 mode. Taper 1, located after the y-splitter, narrows the waveguide to a width of about \SI{250}{\nano\meter} to filter out the TE2 mode, after which the waveguide width is adiabatically increased to 600 nm. The QD is located in a \SI{600}{\nano\meter} wide waveguide region, as marked in this figure, near the center of the waveguide where it couples to both the TE0 and TE2
mode with $\beta\approx0.5$, as shown in Figure \ref{fig:App_betaAndEta}. Any emission into the TE2 is filtered out by Taper 2, which is located before the output coupler, so that we detect predominantly signal from the fundamental mode.

\begin{figure}
\includegraphics[width=11.5cm]{SEM}
\caption{The photonic device, consisting of in/output couplers, a photonic crystal waveguide and tapers. The position of the QD is marked by the yellow circle and the  transition dipole orientation by the arrow. Both the nanobeam waveguides and photonic crystal are suspended, with the former being supported by tethers.  \label{fig:App_SEM}}
\end{figure}

\section*{Resonant transmission formulas}\label{App:Transmission}

\newcommand{s_-}{s_-}
\newcommand{s_z}{s_z}
\newcommand{\gamma_\mathrm{wg}}{\gamma_\mathrm{wg}}
\newcommand{\gamma_\mathrm{rad}}{\gamma_\mathrm{rad}}
\newcommand{\gamma_{d}}{\gamma_{d}}
\newcommand{\gamma}{\gamma}
\newcommand{\Delta\omega}{\Delta\omega}

To derive the transmission spectrum of coherent light through the waveguide with an embedded QD we closely follow the theory in Refs.~\citenum{Javadi2015supp,Auffeves-Garnier2007supp}, which considers the transmission of light through a two-level system in a weakly-coupled optical cavity. We here recap the relevant equations and derive an analytical expression for the full transmission spectrum, which accounts for both the coherently transmitted light under weak excitation and the incoherent part under higher power.

In the studied waveguide weak reflections at the terminations result in a low-Q cavity that modulates the spectral response of the nanobeam waveguide. The bare transmission coefficient through the cavity without the QD is
\begin{equation}\label{eq:App_t0}
 t_0 = \frac{1}{1+\frac{i(\delta-\Delta\omega)}{\kappa}}\approx \frac{1}{1+i\xi},
\end{equation}
where $\Delta\omega = \omega-\omega_0$ is the detuning between the laser frequency $\omega$ and the QD transition frequency $\omega_0$ and $\delta$ is the detuning between the QD and the cavity resonance. Since the QD linewidth is much narrower than the cavity linewidth $\kappa$, we approximate the detunings in the denominator with a single phase factor $\xi$ varying over the narrow scanning range around the QD resonance.

The following equations are written in angular frequency $\Delta\omega$ and decay rates $\gamma$ in units of \si{\per\second} and can be converted to frequency through $\Delta\nu = \Delta\omega/2\pi$ and $\Gamma = \gamma/2\pi$. The coupling between the QD and the waveguide is quantified by  $\beta=\gamma_{wg}/(\gamma_{wg}+\gamma_{rad})$ that describes the collection efficiency of photons into the detected waveguide mode that is scattered from the QD. Here $\gamma = \gamma_{wg}+\gamma_{rad}$ is the total decay rate of the QD and  $\gamma_{wg}$ and $\gamma_{rad}$ is the decay rate into the waveguide mode and other radiation modes, respectively. The electric field amplitude of the transmitted $a^r_\mathrm{out}$ and reflected $a^l_\mathrm{out}$ output fields are related to the input field $a^r_\mathrm{in}$ via the coupled mode equations
\begin{align}\label{eq:App_aral}
\begin{split}
a^r_\mathrm{out} &= -t_0 a^r_\mathrm{in} - i\sqrt{\frac{\gamma_\mathrm{wg}}2}t_0 s_-,\\
a^l_\mathrm{out} &= (1-t_0) a^r_\mathrm{in} - i\sqrt{\frac{\gamma_\mathrm{wg}}2}t_0 s_-.
\end{split}
\end{align}
The steady state solution for the expectation values of the atomic operators $\hat s_- = \ket{g}\bra{e}$ and $\hat s_z = (\ket{e}\bra{e}-\ket{g}\bra{g})/2$ can be derived to be
\begin{align}\label{eq:App_smsz}
\begin{split}
s_- & =-\frac{4}{\gamma_\mathrm{wg}}\left(\frac{i\Omega t_0 s_z}{t_0+\frac{\gamma_\mathrm{rad}}{\gamma_\mathrm{wg}}+\frac{2\gamma_{d}}{\gamma_\mathrm{wg}}-\frac{2i\Delta\omega}{\gamma_\mathrm{wg}}}\right),\\
s_z & = -\frac 12\left(\frac{1}{1+\Omega^2/\Omega_c^2}\right)
\end{split}
\end{align}
where the excitation Rabi frequency is related to the input field amplitude $\Omega = a^r_\mathrm{in}\sqrt{\gamma_\mathrm{wg}/2}$ and the critical Rabi frequency is
\begin{equation}\label{eq:App_Omegac}
 \Omega_c^2 = \frac{\abs{-2i\Delta\omega +(\gamma_\mathrm{rad}+t_0\gamma_\mathrm{wg}+2\gamma_{d})}^2[\gamma_\mathrm{rad}+\gamma_\mathrm{wg}\operatorname{Re}(t_0)]}{8\abs{t_0}^2[\gamma_\mathrm{rad}+2\gamma_{d}+\gamma_\mathrm{wg}\operatorname{Re}(t_0)]}.
\end{equation}

The transmission and reflection coefficient can now be calculated by
\begin{align}\label{eq:App_rtShort}
\begin{split}
t = \frac{\langle a^r_\mathrm{out}\rangle}{\langle a^r_\mathrm{in}\rangle},\\
r = \frac{\langle a^l_\mathrm{out}\rangle}{\langle a^r_\mathrm{in}\rangle},
\end{split}
\end{align}
which for the general expression for the transmission coefficient gives
\begin{align}\label{eq:App_t}
t = \frac{t_0^2\beta\gamma}{(1+n_\tau/n_c)[\gamma+(t_0-1)\beta\gamma+2(\gamma_{d}-i\Delta\omega)]}-t_0.
\end{align}
We have here inserted the $\beta$-factor and introduced the number of photons in the input field per lifetime of the emitter $n_\tau =2(\Omega/\gamma_\mathrm{wg})^2$ and the correspondingly critical photon number $n_c =2(\Omega_c/\gamma_\mathrm{wg})^2$. Using these definitions together with Eq.~\eqref{eq:App_Omegac} we can calculate the critical photon number for a QD on resonance with the cavity ($\delta = 0$) and at the transmission minimum ($\Delta\omega=0$)
\begin{equation}\label{eq:App_nc}
 n_c = \frac{1+2\gamma_{d}/\gamma}{4\beta^2}.
\end{equation}

The transmission in Eq.~\eqref{eq:App_rtShort} and \eqref{eq:App_t} only account for the coherently transmitted light valid under weak excitation. At higher powers incoherent emission from a finite excitation of the QD contributes to the transmitted intensity, which can be calculated as
\begin{equation}\label{eq:App_Pincoh}
\frac{P_\mathrm{incoh}}{{a^r_\mathrm{in}}^2} =1-\left(\abs{t}^2 + \abs{r}^2 + \frac{\gamma_\mathrm{rad}\abs{\langles_-\rangle}^2}{\langle a^r_\mathrm{in}\rangle^2}\right),
\end{equation}
using that the total scattered and emitted intensity has to add to one. The last term account for coherent scattering into other modes than the waveguide mode of interest.
The total normalized transmission is then given by
\begin{equation}\label{eq:App_Tshort}
 T = \left(\abs{t}^2+\frac{\beta P_\mathrm{incoh}}{2\langle a^r_\mathrm{in}\rangle^2}\right) \frac{1}{\abs{t_0}^2}
\end{equation}

Evaluating Eq.~\eqref{eq:App_Tshort}, we arrive at an analytical expression for the full transmission spectrum where $\xi$ acts as Fano parameter that modifies the shape of the spectral response
\begin{equation}\label{eq:App_Tfull}
 T= \frac{[(\gamma+2\gamma_d)((\beta-1)^2 \gamma+2\gamma_d)+4\Delta\omega^2](1+\xi^2)}{(\gamma+2\gamma_d)^2+4\Delta\omega^2+4\beta\gamma\Delta\omega\xi+\left[((\beta-1)\gamma-2\gamma_d)^2+4\Delta\omega^2\right]\xi^2}.
\end{equation}
In the limit of $\xi\rightarrow 0$ the transmission converges to a simple Lorentzian
\begin{equation}\label{eq:App_Tfinal}
 T = 1+\frac{(\beta-2)\beta\gamma(\gamma+2\gamma_{d})}{(\gamma+2\gamma_{d})^2+4\Delta\omega^2},
\end{equation}
where the minimum transmission depends on the $\beta$-factor and the relative dephasing rate (see Eq.~\eqref{eq:T} in the main text) and in the ideal case ($\beta=1$, $\gamma_{d}=0$) the transmission is zero at the QD transition frequency. Equation~\eqref{eq:App_Tfinal} reduces to Eq.~\eqref{eq:T} in the main text for zeros detuning ($\Delta\omega = 0$) after converting from rates to frequencies ($\Gamma =\gamma/2\pi, \Gamma_d = \gamma_{d}/2\pi$).

\section*{Analysis of Power Series}\label{App:PowerAnalysis}
We here describe the analysis of the power series in Figure~\ref{fig:f3_PowerSeries} in the main text. Each transmission spectrum in the power series is fitted with Eq.~\eqref{eq:App_Tfull} from which we extract the minimum transmission, the linewidth, and the Fano factor $\xi$. The Fano factor is nearly power independent with a mean value of $\bar\xi = 0.16$ and a standard deviation of \num{0.05}. The power dependence of the transmission minimum and linewidth can be described by Eq.~\eqref{eq:T} and \eqref{eq:linewidth} in the main text, respectively. Due to the residual peak, the transmission minima are more reliable than the linewidth at high power, i.e. we fit only the transmission data. We fix the relative dephasing rate at the value obtained from Figure~\ref{fig:f2_RFnRT}(c) in the main text and extract an effective $\beta = \num{0.42\pm 0.01}$ and find that the critical power is obtained for an input power of $P_\mathrm{in,c} = \SI{13.1}{\nano\watt}$ coupled into the cryostat. Here the $\beta$-factor is treated as an adjustable parameter since the multi-mode nature of the waveguide led to a sensitivity to the alignment/polarization of the collection grating resulting in contributions from higher order modes that are not well coupled to the QD. The power series was extracted under slightly different and less ideal polarization conditions than the low-power data, thus explaining the increase in the minimum transmission.

We can use the extracted parameters to calculate the coupling efficiency of input light into the waveguide mode by the use of Eq.~\eqref{eq:nc} in the main text. The number of photons in the waveguide per lifetime $n_\tau$ is proportional to the applied optical power $P_\mathrm{in} \alpha = \hbar\omega n_\tau\gamma$ where the coupling efficiency $\alpha$ accounts for the transmission through the microscope objective, the efficiency of the input grating, and the waveguide propagating loss. Inserting $\beta$ and $\gamma_{d}$ into Eq.~\eqref{eq:nc} we obtain the number of photons per lifetime  $n_c = 1.6$ corresponding to an average of $P_\mathrm{wg,c} = \hbar\omega n_c\gamma = \SI{1.88}{\nano\watt}$ traveling in the waveguide. The total coupling efficiency is therefore $\alpha = P_\mathrm{wg,c}/P_\mathrm{in,c}=0.14$, where the dominating loss mechanism is the incoupling efficiency through the circular grating.

\section*{Temperature Dependent Frequency Shift}\label{App:TempDep}

The temperature dependence of the resonance frequency of the QD is shown in the inset of Figure~\ref{fig:f4_Temperature} in the main text. The overall red shift at higher temperatures can be reproduced by a heuristic model of the temperature-dependent band edge shift of bulk semiconductors~\cite{ODonnell1991}, while a minor blue shift is observed at smaller temperatures.
\begin{equation}
	E_g(T) = E_g(0) + \eta \langle\hbar\omega\rangle \left[ \coth(\langle\hbar\omega\rangle/2kT)-1\right].
\end{equation}
From this fit we extract an average phonon energy $\langle\hbar\omega\rangle = \SI{6.6}{\milli\electronvolt}$ and a coupling parameter $\eta=0.48$, whose difference to literature values\cite{ODonnell1991} we mainly attribute to the difference in materials used and that we consider a bound state rather than a bulk material.

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\bibitem[Rotenberg \latin{et~al.}(2017)Rotenberg, T\"{u}rschmann, Haakh,
  Martin-Cano, G\"{o}tzinger, and Sandoghdar]{Rotenberg2017}
Rotenberg,~N.; T\"{u}rschmann,~P.; Haakh,~H.~R.; Martin-Cano,~D.;
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  Hansen}, Midolo, Mahmoodian, Kir{\v{s}}ansk{\.{e}}, Pregnolato, Lee, Song,
  Stobbe, and Lodahl]{Javadi2015supp}
Javadi,~A.; S{\"{o}}llner,~I.; Arcari,~M.; {Lindskov Hansen},~S.; Midolo,~L.;
  Mahmoodian,~S.; Kir{\v{s}}ansk{\.{e}},~G.; Pregnolato,~T.; Lee,~E.~H.;
  Song,~J.~D.; Stobbe,~S.; Lodahl,~P. \emph{Nat. Commun.} \textbf{2015},
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  Simon, G{\'{e}}rard, and Poizat]{Auffeves-Garnier2007supp}
Auff{\`{e}}ves-Garnier,~A.; Simon,~C.; G{\'{e}}rard,~J.-M.; Poizat,~J.-P.
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  2924--2926\relax
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redpajama_set_name: RedPajamaArXiv


The Power Kit includes: 1 traditional #13 thick tube with a larger internal diameter for those who require higher volume or gain. 1 EarHook Adapter to connect to the thick tube. Assorted sizes of closed domes.
The tubing must be trimmed prior to use. See the User Manual for Instructions.
The Kit may be used for either the Left or Right ear.


Probabilistic model-checking (PMC) is a new frontier in model checking verification, useful for checking randomized algorithms, communications protocols with random components, etc. AI techniques have been incorporated into conventional model-checking, with great success. We wish to see if corresponding successes can be found by applying AI techniques to PMC. In this position paper, we introduce PMC. We present the probabilistic automata and probabilistic bounded LTL used in modeling for PMC. We also introduce some existing tools for PMC. With this background in place, we dis- cuss challenges and opportunities for incorporating AI techniques in PMC, and our current work in the area.


text:
extreme legibility
in which peter cameron attempts to remember books he's read before he forgets them
« | Main | »
Moise and the World of Reason by Tennessee Williams
(Simon and Schuster, 1975)
This odd novel was written toward the end of Williams' life (he died in 1983) when he was struggling with drugs and alcohol and trying to regain his literary prowess and stature. Like Albee, he was thought to have lost his talent and genius and anything he produced was ridiculed and dismissed (unlike Albee, he did not live long enough to resuscitate his career and artist reputation). He did produce inferior work during this period, but much of it, like this book and The Two Character Play (1973; see above) contains passages that are heartbreakingly brilliant and beautiful.
Moise and the World of Reason (which is a terrible title--odd for TW, who was so usually so good with titles, especially early on--and does the book a real disservice) is narrated by a 30-year-old man living in a partitioned room in a huge unheated warehouse on the Hudson River at 11th Street. He is an unsuccessful writer who keeps his piles of rejection letters in the crate that he uses as his desk. His first lover, a Black figure skater, has died and he now lives with a younger lover, but they both seem to be biding their time.
The novel takes place over a single day and night. The narrator and his young lover attend a party at their friend Moise's one-room apartment on Bleecker Street. Moise is an enigmatic and waifish painter who specializes in paintings that appear to be unfinished. At the party she announces that she is withdrawing from "the world of reason" and the narrator's lover runs off with another man for dinner at Phebe's (which still exists, having miraculously survived the gentrification of the East Village). The narrator returns to the warehouse and spends the entire night writing in his Blue Jay notebooks, and when he has filled his last one, he resorts to writing on the backs of his rejection letters and on shirt cardboards (which is something James Ivory also does). He writes about growing up queer in Selma, Alabama and running away to the New York City when he was 15, meeting the figure skater, who referred to himself as "the nigger on ice," and their symbiotic friendship with Moise. A few visitors interrupt his writing marathon, and the book concludes with him returning to Moise's room where they seem to be fated to live together in an unworldly darkness and silence (the one window in her room has frosted glass).
Parts of this book are funny, engaging, and written with Williams' poetic flair. His recollections of his mother and grandmother and his figure skater lover are particularly vibrant and fun to read. He writes frankly and graphically about sex and human bodies--it's as is if he making up for all the suppression and inversion in his great plays, and some of the language and acts described are shocking, and must have been extremely offensive to readers in 1975. The New York Times review of this book is a snide, mean, homophobic dismissal, and reading it one feels the derision piled upon Tennessee Williams during this late period. It's sad.
Another interesting thing about this book is its accurate and highly detailed evocation of New York City c. 1975. Williams uses real names of places (Phebe's, The Factory) and people (Warhol, Mary McCarthy, Jane Bowles) and this gives the book a gritty specificity I recognized in the city as I first encountered it in the late 70s and early 80s.
Note: the image above is the cover a New Directions edition of the book, reissued in 2016. I read the original Simon and Schuster edition, pictured below.

redpajama_set_name: RedPajamaCommonCrawl


All but 5% of the participants taking the stress-inducing test showed signs of stress, demonstrated by an increase in cortisol. Overall, 26 percent of all the observers also experienced "empathetic stress," just from watching their partner take the test. As you would probably expect, there was a big discrepancy between the romantic and strange couples.


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Posted on March 6, 2016 March 6, 2016 by Richard Wagner
Pell case: Pontifical Commission calls for prompt response from those in positions of authority
The Pontifical Commission for the Protection of Minors headed by Sean O'Malley, has issued a statement in light of the fracas between Peter Saunders and Cardinal George Pell
Cardinal Sean P. O'Malley of Boston, head of the Pontifical Commission for Child Protection
The Pontifical Commission for the Protection of Minors headed by US cardinal Sean O'Malley, has intervened with a statement in light of the recent clash between Peter Saunders, a member of the Commission who was abused by a paedophile priest when he was a child and Australian cardinal George Pell, Secretary of the Vatican Secretariat for the Economy.
Speaking on Channel Nine's 60 Minutes Australia programme, Saunders accused Pell of showing indifference to the victims of a paedophile priest in Australia when he was a young priest, even going as far as to define Pell's attitude "sociopathic" and expressing the hope that the Pope would remove him from his Vatican role. The prelate – who will be giving evidence at a hearing before the Royal Commission of Inquiry into Institutional Child Sex Abuse after already speaking in a parliamentary inquiry in Victoria – was defensive in his response: he stressed that he never covered up any complaints made against paedophile priests and said he would resort to legal action. The Vatican spokesman Fr. Federico Lombardi also issued a comment, saying that the statement made in recent days by Cardinal Pell in response to the accusations made by the Australian Commission, was "worthy of respect and attention". The Vatican spokesman added that the statements made by Saunders "were clearly entirely personal and were not made on behalf of the Commission". Now, the Commission Saunders is a member of has also expressed itself.
"The Pontifical Commission for the Protection of Minors, as mandated by the Holy Father, Pope Francis, has no jurisdiction to comment on individual cases or inquiries," the statement issued yesterday evening reads. "Regarding Australia's Royal Commission of Inquiry into Institutional Child Sex Abuse, all appropriate questions are being dealt with by the Truth, Justice and Healing Council in Australia, which is coordinating the local Church's response to the Royal Commission's findings," the statement says. "The Pontifical Commission for the Protection of Minors remains dedicated to its mission as outlined in the recently approved provisional Statutes, which is to help the Church worldwide protect minors and make certain that the interests of abuse survivors and victims' are paramount. To this ends the Commission considers it essential that those in positions of authority in the Church respond promptly, transparently and with the clear intent of enabling justice to be achieved."
CategoriesAbuse of Power, Clergy Sex Abuse, Priests In Trouble TagsAvoiding Corporate Responsibility, Catholic Church, Catholic Hierarchy, Catholic Priests, Clergy Abuse Survivors, Priest Abusers
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Whether curled up asleep, tearing around the house or climbing the curtains, kittens are undeniably cute. But don't forget, they are totally dependent on you to provide for their health and well-being to grow into healthy adult cats.A proper diet, vaccination and worming programs, kitten kindy, fighting fleas, de-sexing and micro-chipping are all issues you need to know about. Don't worry. Your best ally will be the team at Vet Cross who will be happy to give you advice on all aspects of your kitten's health.
Kittens need to be vaccinated with the first F4 at 6 to 8 weeks with a booster at 12 weeks. The F4 vaccination protect against Feline Enteritis, Feline Calcivirus, Feline Chlamydia and Cat Flu.
Another vaccination that your vet will advise is for Feline AIDS, commonly known as FIV (Feline Immunodeficiency Virus), and it is spread by cats fighting. It is administered as an initial series of three doses, two weeks apart and is given to kittens at 8 weeks of age or older. Cats more than 6 months of age should be tested to ensure they are free of the AIDS virus before being vaccinated and ideally they should be permanently identified with a microchip. An annual booster is needed to ensure continued protection.
Kittens require these boosters since maternal antibodies obtained from their mother interfere with response to vaccination.
Gastrointestinal worms are dangerous to your kitten's health. Most kittens are infected early in life, especially with roundworms through their mother's milk. Kittens should be wormed at 6, 8 and 12 weeks of age, then every 3 months. Pregnant and nursing queens should also be treated.
Various worming tablets, drops and pastes are available. Recently released is the first spot-on worming preparation that kills roundworms, hookworms and tapeworms in cats. 'Profender' can be used on kittens from 8 weeks of age.
Heartworm disease is not as prevalent in cats as it is in dogs, as the cat's immune system is able to eliminate most infections. However, not all infections are eliminated after the mosquito carrying the immature heartworm bites the cat, and these immature stages can develop to become large worms in the heart and vessels in the lungs. Signs of heartworm disease in cats are variable, and include sudden death. Heartworm disease can be prevented by giving monthly medication, either oral or as a topspot preparation. Ask your veterinarian about the prevalence of heartworm disease in your area.
Kittens have specific requirements for different nutrients, and it is important to feed a high quality, balanced kitten food in order to meet these needs. Dry and tinned forms are available, and they are only different forms of the same food. Most kittens can eat the dry food by 8 weeks of age. If they are eating a balanced kitten food, they require no other supplements, including milk. In fact, some cats have lactose intolerance and develop diarrhoea if given milk.
It is important to train your kitten to eat raw chicken wings and necks from a young age. This is to keep their teeth and gums healthy throughout life. Give them the wing tips first, although most kittens are happy to tackle the whole wing. Periodontal disease is an important disease of middle-aged to older cats, and training your kitten to chew chicken bones from the start will help your cat avoid developing this potentially life-shortening disease.
It is recommended to give a chicken wing at least twice a week. After 12 months, raw bones can be given daily and in increasing amounts to make up to 40-50% of the diet, reducing the amount of commercial food required. Raw lamb cutlets, osso bucco cuts, beef spare ribs or lamb shanks are also good for variety. Chicken wings must be fed fresh and handled as for human consumption to avoid bacterial contamination and food poisoning. Discard any uneaten bones after 1 hour. If you do not wish to feed bones, train your kitten to enjoy tooth brushing from an early age.
Speying your female kitten, and castrating your male kitten, will prevent any unwanted litters, as well as undesirable behaviours. Male kittens can start spraying inside the house to establish their territory from about 6 months of age, and will fight and roam to satisfy the natural male urge to become dominant in their territory. Female kittens first come into season from 5 months of age, and vocalise and become restless when on heat. Breeding from your pet cat is strongly discouraged, since there are so many thousands of cats and kittens put down each year due to cats not being desexed.
To avoid these problems desexing of both males and females is recommended before the onset of puberty, generally around 5 – 6 months of age. Some vets will recommend earlier desexing from 12 – 16 weeks of age. It is best to ask your own vet and be guided by their preference.
There are many different flea preparations available, some of which are combined with other parasite control. Early treatment is recommended since fleas reproduce at astounding rates. Ask your veterinarian for the most appropriate flea control for your kitten.
It is highly recommended to microchip your pet as microchips provide a permanent form of identification that cannot be changed or removed and this identification lasts for the life of your pet. Most will have been micro-chipped by the breeder, but if not, it can be done in a consultation with your veterinarian. The microchip is the size of a grain of rice and is implanted by giving it through a needle, as an injection, beneath the skin between the shoulder-blades. The number on the microchip is then registered with your local council on the Companion Animal Registry. There is also a national database called the Australian Animal Registry, and you can register your cat on this database as well.
Pet Insurance offers you peace of mind. If your pet is involved in an accident or suffers a sudden illness the medical costs can be several hundreds to thousands of dollars.
Unfortunately, many pets are euthanased each year as owners are unable to meet these unexpected costs. Pet Insurance is your safeguard against this outcome.


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Virginia Districts Ask for Legislative Break on Testing ELLs
By Mary Ann Zehr — March 14, 2007 2 min read
It may turn out to be merely a symbolic move, but on behalf of several Virginia school districts resisting a federal mandate to change how they test English-language learners, the Virginia School Boards Association has asked Virginia's senators to introduce legislation in the U.S. Congress that would ensure they would not have to carry out the mandate this school year.
Frank E. Barham, the executive director of the Virginia School Boards Association said in a phone interview that earlier this month, his organization sent a letter asking Sen. John Warner, a Republican, and Sen. Jim Webb, a Democrat, to introduce legislation that would apply to all U.S. school districts with the following language:
"[English-language learners] will be tested under current Title III provisions to determine level of English proficiency. Only when students are deemed sufficiently proficient in English will states be required to adhere to the Title I provisions and administer the federally approved grade level reading test. This emergency revision of the current ESEA (also known as NCLB) is effective only until full re-authorization of ESEA is completed."
It doesn't seem that the two Virginia senators have spent much time considering the request for them to introduce this legislation. The press secretary from Sen. Warner's office didn't return my calls seeking comment on the issue, and Jessica Smith, the communications director for Sen. Webb, said she didn't think he'd received the letter from the Virginia School Boards Association.
The Virginia School Boards Association also sent a letter to its counterparts in other states, asking those associations to join a coalition seeking congressional relief from the mandate concerning English-language learners and testing.
The school board of Manassas City, which had resisted the mandate, changed its position after the U.S. Department of Education made it clear it would enforce the requirement by withholding federal funds. The Manassas board agreed to comply this school year, according to a March 1 article in the Washington Post. But other school boards that initially passed resolutions indicating that they would resist the mandate haven't yet followed suit.
In an earlier post, I mentioned that officials of the Virginia Department of Education have backed down from defending the resisting school districts and agreed to help carry out the federal mandate.
Tom Mendez, a member of the Harrisonburg City school board, told me in an e-mail message that his school board plans to meet with Virginia's senators and representatives in Washington at the end of the month to continue to try to make the board's case in opposing a change in testing this school year. "We're far from giving up the fight for our kids," he said.
When I checked by telephone this week with Paul Regnier, a spokesman for Fairfax County schools, he said the Fairfax County school board hasn't yet made a determination of how it will carry out testing for English-language learners this spring, given recent developments.The resolution passed by Fairfax County schools doesn't explicitly say that the district will resist the federal government's mandate, he noted, but rather that "we will continue to test our LEP kids with the appropriate testing."
Mary Ann Zehr
Mary Ann Zehr was an assistant editor for Education Week. Her beats included English-language learners, bilingual education, immigrants, dropouts, achievement-gap issues, and charter and private schools. She is the author of the blog Learning the Language.
A version of this news article first appeared in the Learning the Language blog.


It refers to a reddish brown color like the suzume's (meaning sparrow in Japanese) head.
The dying technique has been employed in China from the ancient times.
However, it seems that the Chinese suzumecha turns out to be darker than the Japanese suzumecha.
There is no written record on this color from the Edo Period in Japan.
This color seems to have emerged after the Meiji Period.