Common and widespread at low and middle elevations throughout four-county area. Nests generally below 3,000 feet in variety of habitats, including forest clearings, orchards, wetlands, bogs, riparian corridors, parks, and neighborhoods. Requires small trees for nesting adjacent to suitable foraging opportunities for berries and insects. Prefers deciduous growth, so may be increasing in residential areas where ornamental tree plantings have replaced conifer forest. Utilizes Russian olive groves in Kittitas County, but absent from much of steppe zone. Transient birds well into June may skew true breeding distribution.


Last month saw the introduction of Feioi Finds – a curated collection of some lovely wish-list-worthy items for your viewing pleasure. I was falling for some gorgeous mirrors in May and this month I'm turning my attention to the great outdoors.
Who doesn't love a good BBQ? We certainly do in our house, and it's so lovely to spend time outdoors when the weather is good enough. As darkness descends on a cool summer's eve, there's nothing like a blazing fire to keep the party going. Just because the sun has gone to bed, doesn't mean we have to! We've been shopping around for fire bowls and baskets so I thought I'd use the opportunity to share my #FeioiFinds with you!
Designed by the ultra cool designers at House Doctor in Denmark, this stylish fire bowl rests on a three-legged stand. The simple yet elegant piece is ideal for contemporary gardens and complements Scandinavian style homes. Available from Grace & Glory for £265.00.
We're sticking with the Scandi theme for now with this striking design by Norm Architects for Menu. Formed out of black oxidised steel – which is stronger and more durable than cast iron – the modern fire basket is a unique centrepiece for indoors and outdoors. Fill with logs for fireside storage during the winter months and bring outdoors to enjoy toasty fires on cool summer evenings. Available from Black by Design for £149.95.
You may remember the Solus Decor Hemi 36″fire bowl from my Inside out post. It's a little on the pricey side but such a stunner, I had to include it again. Available with a natural gas / LPG or bio fuel burner and with both manual and electronic ignition, the huge concrete bowl will pump out some serious heat. As well as looking incredible, it's totally fuss free without having to faff around with logs and kindling. The top can be protected with an all-weather cover but there's also the option to purchase a wooden top to convert it into a table when not in use as a fire bowl.
This unusual design by Ak47 Design is the Tripee fire pit from Houseology. "What the hell is a Tripee?" I hear you ask. Is it a cross between a tripod and a teepee? Who knows? In this case it's a beautiful steel fire bowl suspended within an elegant tripod. Currently reduced from £1,540.00 on Houseology.
So, which one did we go for?
Its neat size makes it perfect for our garden and I love the shallow curve of the bowl allowing the fire to be visible from all angles. It's made of cast iron making it reassuringly weighty and giving the appearance a rustic charm.
Fancy your own fire bowl or basket to add to your outdoor space? Which one is the one for you?
Unfortunately the weather is not playing ball at the moment so we haven't had a chance to use ours yet. I'll be waiting patiently for a lovely summer evening to relax around a fire. All you need are marshmallows and your best ghost stories. Who's with me?
Don't forget to leave me a comment if you have a suggestion for next month's Feioi Finds post!
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Check out the latest collection from Julien Macdonald for Debenhams Home.


The South Dakota Game, Fish and Parks (GFP) has documented the first deer mortality in 2016 due to hemorrhagic disease, also known as epizootic hemorrhagic disease (EHD) or blue tongue. EHD was recently confirmed by laboratory analysis in a white-tailed deer in the southeastern part of the state.
The virus is spread by a biting midge and causes extensive internal hemorrhaging. Many deer exhibit no clinical signs and appear perfectly healthy, while others may have symptoms such as respiratory distress, fever and swelling of the tongue. With highly virulent strains of the virus, deer can be dead within one to three days. Affected deer are often found near low lying areas or near water like a river or a pond. This is due to the deer going to water to combat the high fever.
As there will be a heightened level of activity on the country-side during crop harvest and hunting seasons, GFP asks anyone who observes sick deer or finds several dead deer to contact their local conservation officer or local GFP office. This information is valuable to wildlife managers in monitoring deer populations across the state.
EHD outbreaks can be locally severe, but rarely affect a high proportion of a deer population. In rare cases, the disease can affect deer populations in certain areas of South Dakota as observed in 2012 and 2013. License adjustments were made in some units to react to these unforeseen mortality events. Deer can continue to succumb to this disease until a hard freeze reduces midge populations that carry the disease.


This item is incompatible with Sid Meier's Civilization: Beyond Earth. Please see the instructions page for reasons why this item might not work within Sid Meier's Civilization: Beyond Earth.
Retrograde thrusters now allow you to choose a start point within a six square radius instead of 2.
Does this work with RT?
Hello, could you please post link for external download?
Cna anyone help me PLZ. I have dowloaded this Mod but it doesn't work! I am a noob to this sorta thing!
@cloud9landscape If your using the SQL update, you need to make sure in your mod properties you add an "OnModLoad" -> "UpdateDatabase" -> "with your file" action.
@PAC there is a variable for changing the "vision" range, but my game crashed whenever I touched it.
Is there any way to change the start "vision" range granted by retrograde thrusters?
I play on the Massive map myself but I'd still prefer 4. Big thanks for the tip to user change it by the way.


The compact flowsensor SNS 552 measures the flow of water based media and displays the measuring values (liter or m³) in the display. Furthermore the sensor delivers the temperature values from 0…80 ° C. The sensor provides two outputs: optionally two switching outputs (normally closed, normally open), analog outputs or switching output and analog output.
The SNS 552 is insensitive against temperature changes and features a fast reaction time. For processes with frequently changing liquids the sensor delivers a teach in mode for instant online setup for new components. The rotable Display provides a good readability of the values from all directions.
The sensor is parametrized using the front buttons or the IO-Link interface. With IO-Link it is furthermore possible to integrate the sensor easily in any common bus-system.


text:
December Seniors Named at H. Frank Carey
H. Frank Carey has recognized Saher Shafiq and Joseph Savoretti as Seniors of the Month for December.
Saher is engaging, respectful, considerate and a genuinely kind person. Her thirst for knowledge, natural intellect and desire to learn is unmatched. Saher's maturity is evident in every endeavor that she undertakes. Academically, this AP Scholar with Honor student is ranked in the top of her class, and her achievements have been recognized by nomination and acceptance into the English, National and World Language honor societies. She has held several leadership positions as president of Art Palettes, president of 21st Century Scholars, editor of the yearbook, president of Saving Our Society, president of the Desi Society, a contender in the Mathletes, managing editor for Carey Clipper and editor-in-chief of the Poseidon Literary Magazine. Additionally, she is extremely active in community service, speaks five languages and has many achievements in local science fairs and competitions. This senior has applied to a wide range of colleges and universities that include a mix of Ivy League and other highly selective programs.
Joseph is a warmhearted person who shows nothing but sincerity and kindness to those around him. He has demonstrated hard work and perseverance in all subject areas, evident by his acceptance into the National Honor Society as well as the National Technical Honor Society. Joseph stands out in a sea of high-achieving students not only for his academic standards, but for his character and demeanor. This young man is extremely active in school activities as treasurer of the Student Government and student representative for the Class of 2019 Board. He has been a longtime member of the Boy Scouts of America and has earned the prestigious rank of Eagle Scout. He is a skilled musician and knows how to play both the trumpet and the drums. Additionally, he is a member of the Instrumentation and Automation vocational program and has competed in several conferences in the Model United Nations. Those around him admire his determination to succeed and how he leads without knowing it, in a subtle, understated way.
Congratulations to Saher and Joseph!

redpajama_set_name: RedPajamaCommonCrawl


You can find a desperation for Him in the knowledge that despite our best laid plans, we cannot predict the future. We can trust our ability to adapt to each days new circumstances, only turning to God for help when our abilities fail us. But there is no greater feeling than realizing you are hopelessly out of control, but that you have the God of the universe on YOUR side and He is.


text:
Joe Mixon 'Frustrated' By Bengals Inability To Run Ball
Wednesday, November 06, 2019 / Gilbert Sam /
John Grieshop/Getty Images
Cincinnati Bengals running back Joe Mixon is 'frustrated' by the team's running ability or lack thereof, only totaling 476 yards of rushing through eight games.
Bengals' first-year head coach Zac Taylor, hoping to kickstart the offense, benched veteran play-caller Andy Dalton in favor of rookie quarterback Ryan Finley over the bye week. The team Is winless after going 6-10 last season under Marvin Lewis.
Mixon, coming off a 1,168-yard performance in 2018, entered the season with expectations of being the league rushing leader. Afterall, Los Angeles Rams' offense ranked third in rushing yards under the direction of then-offensive coordinator Taylor.
"Everybody knows that I'm frustrated. Who wouldn't be frustrated? I feel like I should be putting up way better numbers than what I'm putting up toght now," Mixon said, via the Cincinnati Enquirer.
Mixon has only 320 yards this season, averaging on 3.2 yards per carry.
"To go from first in the AFC in rushing and s–t, we're probably last right now in the AFC. It's embarrassing to me. That's not my expectation and it shouldn't be anybody else's expectation. I'm not complacent to what the hell is going on. I'm frustrated. Everybody knows that I'm frustrated, but the coaches are frustrated, too. We are all frustrated."
The offense has struggled under Taylor ranking 29th in pts per game, 25th in yards per game and a league-worst 32nd in rushing yards per game.
Bengals host division rival Baltimore Ravens on Sunday.


In 2001, I attended a RIPE training in Copenhagen where they showed us the estimated timeline predicting when IPv4 address space would reach depletion. They mentioned the "new and fancy" IPv6 protocol. When I returned from the training, I started to lab with 6Bone and moved over to SIXXS after a while. At this time, we only had one auth DNS and one mailserver with IPv6 capabilities, and only about one mail per month was delivered via IPv6. There was no pressing need for IPv6 this early, except that my employees and I could learn it and make mistakes without any disturbance for us or our customers. The only real content over IPv6 at this time was the the dancing turtle.
In 2007 we received native IPv6 from our ISP (AS16117) and it has worked well since then. My company, Interlan, has been an early adopter of IPv6 for many years and all our internal network and public services are dual-stacked. We work in the middle of the Internet industry as an ISP with hosting and consulting for enterprises. Our opinion is that the Internet can't scale any longer and be secure and stable with IPv4 and more and more NAT44, NAT444, etc.
Make sure the ISP is ready with the setup (e.g. Ping from the inside interface from the firewall to make sure the routing is correct).
Create every firewall policy in advance.
Manually configure servers that need static addresses and let the others use dynamic addresses. In a Windows AD environment it's almost only the DC, DNS and mailservers who need static addresses. The rest can use dynamic address assignment.
When the set-up above is ready and you need it, add some AAAA RR in the DNS to activate IPv6 on public services like a webserver.
You will find out that it isn't hard to make it work if you know your IPv4.
Today, it is extremely important to enable IPv6 correctly. Global IPv6 is about to reach 20% according to Google's measurement, and you can't afford to not be connected to the whole Internet. Hosts, firewall, DNS, etc. must all be done correctly.
In Sweden, we unfortunately have a common problem with broken IPv6 from authorities who think they set it up correctly, but IPv6 doesn't work properly. Even if we have only 4.57% IPv6 in Sweden, that is a huge problem for citizens trying to reach those authorities. The best solution for that kind of problem is to enable IPv6 all the way in the internal network, not only the public servers. Internal users are the best monitors.
Don't be surprised when you see that more than 50% of your Internet traffic will be IPv6.
Remember to have the same security functions for IPv6 as for IPv4. Antivirus, webbfilter, IPS, App control should work for IPv6 as well.
Test your firewall rules, so ICMPv6 PTB can be sent to your webserver.
Disable IPv4 on your workstation and connect to your website to see where there are IPv4 dependencies.
But do you really need dual stack in your enterprise? Can't you use NAT64 instead of NAT44? I wrote an earlier blog here about that. I run default native IPv6 with NAT64 in my office now, and it works consistently, and for a "normal user" there should be no problems at all.
Torbjörn Eklöv is Co-Founder and Owner of Interlan and has been an IPv6 geek since 2001.


text:
\section{Introduction}
Quantum devices based on topological order are expected to be robust against many common forms of decoherence, making them an exciting prospect for quantum computation \cite{Kitaev2001,Kitaev2003,Kitaev2006,Nayak2008,Stanescu2016}. Although originally envisaged as a 2D platform, the realisation that quasi-1D proximity-coupled systems \cite{Fu2008,Lutchyn2010,Oreg2010}
could be employed in network architecture \cite{Sau2010,Alicea2011}  has led to a great deal of theoretical \cite{Duckheim2011,Chung2011,Choy2011,Kjaergaard2012,Martin2012,NadjPerge2013,Aasen2016} and experimental \cite{Mourik2012,Deng2012,Das2012,Finck2013,Churchill2013,Albrecht2016, Zhang2016,Deng2016,NadjPerge2014,Ruby2015,Pawlak2016,Zhang2018} work. However, despite significant advances, the current reality is that devices based on proximity-coupled superconductors still suffer from errors. There is a range of problematic processes that potentially limit the effectiveness of topological quantum memories. The majority of these\cite{Goldstein2011,Budich2012,Rainis2012,Mazza2013, Ho2014, Ng2015,Campbell2015,Pedrocchi2015,Huang2018, Knapp2018, KnappNoise} concern the inevitable interaction with an external environment. However research in this area has also focused on errors due to changes of the internal system parameters over a finite time, e.g., due to fluctuations in the underlying gate potentials \cite{Schmidt2012}, thermal noise\cite{Cheng2012}, or the deliberate shuttling of Majorana-Bound-States (MBS) around a network \cite{Cheng2011,Perfetto2013,Bauer2018,Karzig2013,Scheurer2013,Knapp2016,Rahmini2017,Karzig2015,KarzigShortcut}.

In this work we set out to examine error generation in this latter scenario and analyse how initial qubit-loss error can give rise to additional bit and phase-flip errors.  For idealised topological qubits, any excitations away from the ground state manifold represent a source of qubit-loss error. We examine this issue from the perspective of a simple topological memory constructed from two spinless $p$-wave superconducting wires, connected via a single tunnel junction, specifically studying how qubit-loss depends on (1) time-dependent fluctuations in the confining potentials and (2) the non-adiabatic transport of Majorana bound states.

Our analysis in the case of oscillating boundary walls indicates that the frequency dependence of the error rate is strongly correlated with the local density of states at the edge of the wire.  We also find that the maximum coupling to bulk states is inversely proportional to the bulk gap, but that the frequency at which this maximum coupling occurs increases as we increase the superconducting gap. For the very low frequency oscillations this naturally coincides with the expected behaviour in the adiabatic limit. However on the high-frequency side we see that this can mean a reduction in qubit stability as the bulk gap is increased.

On the question of Majorana bound state transport, significant progress has been made previously by Refs. \onlinecite{Karzig2013,Scheurer2013} where it was shown that MBS can be transported without incurring any significant qubit loss, provided that the acceleration is sufficiently slow and the maximum velocity is less than a critical value. Our findings here are mostly in agreement with these previous works. However, we observe no advantage in keeping the wire's length fixed during a movement protocol, a  departure from previous predictions in relation to correlated movement of distant boundary walls outlined in Ref. \onlinecite{Scheurer2013}.
Our results also show that it is possible to think of  the instantaneous energy increase as a kinetic energy of the boundary wall, with an effective-mass $ M^* \propto k_F / 2 \Delta= k_F^2/2 E_{\text{gap}}$, that incurs relativistic-like corrections when it approaches the critical velocity. We also show that there is only a modest additional qubit-loss penalty for approaching the infinite acceleration limit in the $v_\text{max} < v_\text{crit}$ regime\footnote{This feature has been proposed to be used in so called bang-bang control protocols \cite{Karzig2015}.}.

In addition we study how initial qubit-loss leads to secondary error processes such as bit and phase-flip error.  This is important because although qubit-loss the is the primary source of error in this setup, it is in principle detectable (e.g. via a projective energy measurement), and therefore its existence alone does not pose a fundamental problem for the stability of the quantum memory and/or any ongoing quantum computation. In contrast a more damaging situation occurs when the original error is followed by some secondary processes that, after some time, returns the system to the qubit-space with an error. These error processes cannot be detected without some additional error detection/correction protocols, a scenario which topological schemes are supposed to avoid.

\begin{figure}[t]
\centering
 	\includegraphics[width=1\columnwidth]{setup.png}
	\caption{(Colour online) Top: A schematic illustration of the Kitaev chain used to encode a single topological qubit. Majorana bound states (MBS) are localised at the boundaries between topological and non-topological regions. Bottom: The chain is in a topological phase in regions where $|\tilde{\mu}| < 2|w|$ (the shaded area) and in a non-topological phase in regions where $|\tilde{\mu}| > 2|w|$. The MBS at $x_\text{wall}^{(i)}$ is manipulated by moving the boundary wall with a velocity profile $v_\text{wall}^{(i)}(t) = dx_\text{wall}^{(i)}(t)/dt$.}
        \label{fig::setup}
\end{figure}
For bit-flip error our central results are that boundary wall movement will generate localized quasi-particles that can propagate across the wire and cause errors if they tunnel through boundary walls separating topological regions. The times at which the errors begin to appear can be estimated from the velocity of the wave-front, which is approximately equal to the Fermi velocity  $v_f$. We also investigate a possible way to reduce such errors: by inducing disorder in the bulk of the wire, the bulk excitations can be made subject to disorder induced localization, which prevents propagation of the wave without lowering the critical velocity of the system.

We also discuss undetectable phase errors. These could potentially occur in the same manner as the bit flip error, but we actually identify another process through which the qubit may be vulnerable to uncontrolled rotations and which can already occur in a single wire. The error process does not require any non-local effects and/or tunneling between topological domains, but it is dependent on the existence of an energy mismatch between certain bulk eigenstates. In our study, since we restrict ourselves only to non-interacting systems, this error channel is only open when there is some overlap between the edge modes, meaning that they are not strictly zero modes -- a typical finite size effect. This means in particular that we will already have some Rabi oscillations between the qubit states as they are not perfectly degenerate. These expected oscillations can be modified when the splitting of pairs of excited states differs from the qubit states' splitting. A similar error channel may be relevant also when one wishes to deliberately rotate non-topologically within the ground state manifold. In interacting systems, we might expect this type of phase error even if the system size is large enough to make the ground state splitting negligible, since the spectrum is no longer described by single particle modes and energy mismatches between excited states can occur even if the ground state degeneracy is robust.

An outline of the paper is as follows. In section \ref{sect:Overview}, we review the Kitaev model for a $p$-wave superconducting wire and describe how we calculate and analyze the dynamics generated by the movement of boundary walls. In section \ref{sect:QubitLoss}, we discuss the qubit-loss error due to the moving walls. We divide this section into two parts. First, in section \ref{sect:oscillating_Qubit_Loss}, we focus on oscillating boundary walls. Next, in section \ref{sect:Adiabatic_Qubit_Loss} we investigate qubit-loss error due to non-adiabaticity during transport of Majorana bound states (MBS) along a wire. In section \ref{sect:secodaryerrors} we present our results on the secondary processes that can cause bit and phase-flip errors in the computational subspace. We also divide this in two: in section \ref{sect:BitflipError} we discuss bit-flip errors in the two-wire scenarios and in section \ref{sect:phase_error} we discuss phase errors due to non-adiabaticity. Finally, in section \ref{sect:Conclusions} we summarize and discuss possible avenues of future work.

\section{Model}\label{sect:Overview}

\subsection{The Kitaev model}

The Hamiltonian for the Kitaev model of a $p$-wave superconductor is
\begin{align}
\label{eq:Hamiltonian}
	H & = -\sum_{j=1}^{N} \tilde{\mu}_{j} (c^\dagger_{j }c_{j }-1/2) - w \sum_{j=1}^{N-1} (c^\dagger_{j}c_{j+1} + h.c.) \nonumber \\
	& \quad + \tilde{\Delta} \sum_{j=1}^{N-1} ( c^\dagger_{j} c^\dagger_{j+1} + h.c. ) - \sum_{j=1}^{N} \lambda_{j}{c}^{\dag}_{j}c_{j},
\end{align}
where $c_j$ is the fermionic annihilation operator at the $j$'th lattice site, $\tilde{\mu}_{j}$ is the lattice chemical potential, $w$ represents the hopping strength between neighboring lattice sites, and $\tilde{\Delta} \neq 0$ is the lattice pairing parameter, which induces a superconducting gap.

The chemical potential $\tilde{\mu}_j$ can vary across the wire and will be used to control the boundaries between topological regions (where $|\tilde{\mu}_j| < 2|w|$) and non-topological regions (where $|\tilde{\mu}_j| > 2|w|$). Majorana bound states are localised at the boundaries between topological and non-topological regions in the wire. We model a boundary wall separating a topological and a non-topological region -- at a position $x_\text{wall}$ along the wire -- by a sigmoid function for the chemical potential (see Fig.~\ref{fig::setup} for an illustration showing several boundary walls and see Appendix \ref{app::wall} for further details on the boundary wall function). To move a boundary wall we allow the wall position $x_\text{wall}(t)$ to be time-dependent. Equivalently, we can specify a time-dependent wall velocity $v_\text{wall}(t) = dx_\text{wall}(t)/dt$. This results in a time-dependent chemical potential $\tilde{\mu}_j(t)$, and hence a time-dependent Hamiltonian (\ref{eq:Hamiltonian}). Disorder in the chemical potential is introduced using the Gaussian random variable $\lambda_{j}$, which has zero mean $ \langle \lambda_{j} \rangle=0$ and variance $\langle \lambda_{i}\lambda_{j} \rangle = \alpha \delta_{ij}/a$, where $a$ is the lattice spacing.

In order to solve the system, the Hamiltonian (\ref{eq:Hamiltonian}) can be rewritten as $H(t) = \sum_{n=1}^N \epsilon_n(t) [\beta_n^\dagger (t) \beta_n (t) - 1/2]$ via the Bogoliubov transformations:
\begin{equation}
\label{eq::bogoliubov}
\begin{split}
	& \beta_{n}(t) = \sum_{j} U_{j,n}(t) c_{j} + V^*_{j,n}(t) c^{\dagger}_{j},  \\
	& \beta^{\dagger}_{n}(t) = \sum_{j} U_{j,n}^{*}(t) c^{\dagger}_{j} + V_{j,n}(t) c_{j},
\end{split}
\end{equation}
where $U_{j,n}(t)$, $V_{j,n}(t)$ are the coefficients of the unitary matrix that diagonalizes the Bogoliubov-De Gennes (BdG) Hamiltonian associated with $H(t)$. We assume that the spectrum is labeled in increasing order $\epsilon_0 \leq ... \leq \epsilon_{N-1}$. Pairs of Majorana bound states, if well separated, are associated with zero energy modes ($\epsilon_0 \approx 0$, $\epsilon_1 \approx 0$,... etc.). If there are $m$ such zero modes $\{\beta_j\}_{j=0}^m$, then there are $2^m$ degenerate ground states $(\beta_0^\dagger)^{l_0}...(\beta_m^\dagger)^{l_m}|\text{GS}\rangle$, where $l_j \in \{0,1\}$ and $|\text{GS}\rangle$ is the BCS ground state.

We also note that the continuum limit of the chain can be obtained by taking the total number of lattice sites $N \rightarrow \infty$ and the lattice spacing $a \rightarrow 0$, with the length of the wire $L = Na$ kept constant. In this limit, the lattice Hamiltonian (\ref{eq:Hamiltonian}) becomes a low energy effective Hamiltonian
\mbox{$H = \int_0^L \! \! dx\, \Phi^\dagger(x) [(-\partial_x^2/2m \!-\! \mu(x) \!-\! \lambda(x))\sigma_z \!+\! \Delta\partial_x \sigma_x] \Phi(x)$},
where
\mbox{$\Phi^\dagger (x) = (c^\dagger (x) \: c(x))$}.
It will be useful to express some of our results in terms of the continuum parameters $m$, $\mu$ and $\Delta$, which are related to the lattice parameters by $m = 1/(2wa^2)$, $\mu = \tilde{\mu}_{j} + 2w$, and $\Delta = 2a\tilde{\Delta}$. In this limit, the chain is in a topological phase when $\mu > 0$ and in a non-topological phase for $\mu < 0$. Using the continuum parameters, it is also useful to define the Fermi momentum $k_F = \sqrt{2m\mu}$, the Fermi velocity $v_F = k_{F}/m$, the gap energy $E_\text{gap} = \Delta k_F$, and the finite localization length due to disorder $l=v_F^2/\alpha$.

\subsection{The Topological qubit}\label{sec:topo_qubit}

Throughout this paper we consider a topological system that encodes the smallest unit of quantum information, a qubit. If we are restricted to a subspace of fixed fermion number parity, a topological qubit needs at least four Majorana zero modes, and hence two topological regions in the wire, separated by a non-topological region. This is implemented in our model with four boundary walls at the positions $\{ x_\text{wall}^{(1)}, x_\text{wall}^{(2)}, x_\text{wall}^{(3)}, x_\text{wall}^{(4)} \}$ (see Fig.~\ref{fig::setup}). The qubit space is then encoded in either the global even or odd parity subspace of the associated 4-fold degenerate ground state space $\{ |\text{GS}\rangle, \beta_0^\dagger |\text{GS}\rangle, \beta_1^\dagger|\text{GS}\rangle, \beta_0^\dagger\beta_1^\dagger|\text{GS}\rangle\}$.
We will choose our logical qubit to be spanned by the ground states of the even-parity sector $\ket{\bar{0}} \equiv |\text{GS}\rangle$ and $\ket{\bar{1}} \equiv \beta_0^\dagger\beta_1^\dagger|\text{GS}\rangle$. We emphasize that, since the Hamiltonian $H(t)$ can be time-dependent, the spectrum $\epsilon_n(t)$, the normal mode operators $\beta_n(t)$, and the degenerate ground states $\{ \ket{\bar{0}(t)},  \ket{\bar{1}(t)} \}$ can also be time-dependent
\footnote{We note that the notation here could lead to the misconception that the qubit-space is identified with the occupation numbers of the Majorana zero modes alone. This would in turn imply that fidelity measures of the qubit-space can be computed by performing a partial trace over the bulk-eigenmodes.
In the following we will take the view that readout protocols that can distinguish fermionic and vacuum channels (see for example \cite{Aasen2016}) must, in some guise, project to the actual energy eigenstates and as such, should also be able to detect errors that come from states where the occupation numbers of some bulk modes, together with one or both Majorana zero modes, have been flipped.  In this paper we therefore do not see bulk excitations by themselves as an insurmountable problem.
However we are concerned about the damage excitations can do when they, through a variety of mechanisms, find their way back to the ground state manifold.}.
In appendix~\ref{sect:BdG} we outline how excitations and superpositions thereof are handled within the BdG formalism.

In what follows we will need to sometimes specify bulk eigenstates. In this case we will adopt the following notation
\begin{align}
\ket{ 00 \{n_B \}} = \ket{0}_L \otimes \ket{0}_R \otimes \ket{n_B}  \nonumber \\
\ket{ 11 \{n_B \}} = \ket{1}_L \otimes \ket{1}_R \otimes \ket{n_B}
\label{eq:estatenotation}
\end{align}
where $n_{B}$ is binary number encoding the bulk mode $\beta_n$ occupations and the $L/R$ subscript refers to the zero mode of the left/right wire. In this notion our two ground states would be written as
$\ket{\bar{0}} \equiv \ket{ 00 \{0...0 \}}$ and $\ket{\bar{1}} \equiv \ket{ 11 \{0...0 \}}$

\subsection{Dynamics}
At some initial time $t = t_\text{init}$, we suppose that the system is in the state $\ket{\psi(t_\text{init})} = \alpha_0 \ket{\bar{0}(t_\text{init})} + \alpha_1 \ket{\bar{1}(t_\text{init})}$, where $\ket{\bar{0}(t_\text{init})}$ and $\ket{\bar{1}(t_\text{init})}$ are ground states of the Hamiltonian $H(t_\text{init})$ at that time. At a later time $t$, the system has evolved to the state $\ket{\psi(t)} = \mathcal{U}(t,t_\text{init}) \ket{\psi(t_\text{init})}$, where $\mathcal{U}(t,t_\text{init})=\mathcal{T}e^{-i\int_{t_\text{init}}^t H(t')dt'}$. If the boundary walls, and hence the Hamiltonian $H(t)$, are changed very slowly then, by the adiabatic theorem, in the ideal case, the system at a later time $t$ will remain in a superposition of the instantaneous ground states, $\ket{\psi_\text{ideal}(t)} = \alpha_0 \ket{\bar{0}(t)} + \alpha_1 \ket{\bar{1}(t)}$ with the same amplitudes as the initial state. This is the key feature of topological computation: if we assume adiabaticity, the only way to rotate within the ground state space is to ``braid" MBS around each other. We regard $\ket{\psi_\text{ideal}(t)}$ as the ideal, error-free evolution. Deviations from adiabaticity will lead to excitation of the bulk modes, corresponding to qubit loss. We quantify the qubit-loss by the probability $P_\text{loss}$ that the system is not in one of our instantaneous qubit states:
\begin{equation} P_\text{loss}(t) = 1 - \hspace{4pt} |\langle \psi(t) | \bar{0}(t)\rangle|^2 - |\langle \psi(t) | \bar{1}(t)\rangle|^2  \hspace{4pt}.
\end{equation}
This gives $P_\text{loss}=0$ if there is no qubit-loss and $P_\text{loss}=1$ if the qubit is completely lost. Since qubit loss corresponds to energy excitations, qubit-loss errors can, in principle, be detected by projective measurements of energy. More damaging are the undetectable errors resulting from bulk excitation returning to the wrong ground state. We consider two types of qubit error: bit flips and phase flips. A bit-flip error occurs if the system returns to the qubit space in the state $\ket{\psi_\text{bit}(t)} = \alpha_0 \ket{\bar{1}(t)} + \alpha_1 \ket{\bar{0}(t)}$ (i.e., with the qubit basis states exchanged $\ket{\bar{1}(t)} \leftrightarrow \ket{\bar{0}(t)}$). We quantify the bit-flip error with the probability:
\begin{equation} P_\text{bit}(t) = |\langle\psi(t) | \psi_\text{bit}(t) \rangle |^2 . \end{equation}
In the following study of bit-flip error we will generally choose $\ket{\psi(0)}=\ket{\bar{0}}$ and thus the bit flip error is simply given as $P_{\text{bit}} = |\braket{\psi(t)}{\bar{1} (t)}|^2$.

Phase-flip error occurs if the system returns to the qubit state $\ket{\psi_\text{phase}(t)} = \alpha_0 \ket{\bar{0}(t)} - \alpha_1 \ket{\bar{1}(t)}$, with the probability:
\begin{equation} P_\text{phase}(t) = |\langle\psi(t) | \psi_\text{phase}(t) \rangle |^2 . \end{equation}
In the following discussions of phase-flip error we will choose $\ket{\psi(0)} = \ket{\psi_+(0)}\equiv \frac{1}{\sqrt{2}} (\ket{\bar{0}}+\ket{\bar{1}})$ and  $\ket{\psi_\text{phase}(t)} = \ket{\psi_-(t)} \equiv \frac{1}{\sqrt{2}} (\ket{\bar{0}(t)}-\ket{\bar{1}(t)})$.

All the above amplitudes are numerically evaluated using the Onishi formula\cite{Onishi1966,NuclearManyBody2004}. See Appendix \ref{sect:BdG} for more details.

\begin{figure*}[t]
\centering
\includegraphics[width=2\columnwidth]{L200loss_map.pdf}
\caption{(Colour online) (a) The time-averaged qubit-loss, as a function of the wall velocity parameters $v_{\text{max}}$ and $\omega$. The horizontal black line shows the critical velocity $v_{\text{crit}} = |\Delta| = 0.3$. To generate this figure we used $L=200, a=1, m=0.5, v(t) = v_{\text{max}} \sin(\omega t)$, and $\mu = 0.5$. The boundary potentials in this case were set to be essentially infinite ($\mu_{\text{boundary}}=-2000$) and the wall gradient with $\sigma = 1$ (see Appendix \ref{app::wall} for details on wall parameterisation). (b) A cross section of (a) at $ v_{\text{max}} = 0.02$. We see that the maximum qubit-loss rate occurs when the frequency is close to $E_{\text{gap}}$, but where the maximum value decays as $ 1/E_{\text{gap}}$.  The low frequency regime corresponds to the super-adiabatic limit and so we typically see very low rates of qubit loss error. For higher frequencies we see that error rate drops off as  $1/ \omega^4$. Crucially, because the maximum resonant frequency scales with $E_{\text{gap}}$, in the high frequency regime, increasing the topological order parameter can make the system more susceptible to errors.
}
\label{fig:OmegaQubitLoss}
\end{figure*}

\section{Qubit loss}
\label{sect:QubitLoss}

In this section we discuss how the principal source of qubit error (i.e. qubit loss) arises in a simple Majorana wire set-up with moving walls. First, in section \ref{sect:oscillating_Qubit_Loss}, we consider a wall that is oscillating sinusoidally in position. Such a motion may result, for example, from noise in the gates used to control the confining potential, or as a Fourier component of some deliberate wall motion. Then, in section \ref{sect:Adiabatic_Qubit_Loss} we consider a wall that is accelerated to some constant velocity and then, after some time, decelerated back to rest. This corresponds to a scenario where one needs to shuttle Majorana bound states between two different points in space.

\subsection{Qubit-loss due to an oscillating wall}
\label{sect:oscillating_Qubit_Loss}

We first consider the qubit loss $P_\text{loss}$ due to the motion of a single boundary wall, the wall at position $x_\text{wall}^{(1)}$, with an oscillating velocity profile of the form:
\begin{equation}
v^{(1)}_\text{wall}(t) = v_\text{max} \sin (\omega t).
\label{eq:v_wall_osc}
\end{equation}
Since the wall is continuously moving, it is appropriate to calculate the time-averaged rate of qubit-loss \mbox{$\langle dP_\text{loss}/dt \rangle = \frac{1}{t'' - t'}\int_{t'}^{t''} dt (dP_\text{loss}(t)/dt)$}, over a time interval \mbox{$t^{''} - t^{'} = 2n \pi / \omega$} spanning some periods of the oscillation.  The colour map in Fig.~\ref{fig:OmegaQubitLoss}(a) shows $\langle dP_\text{loss}/dt \rangle$ as a function of the wall motion parameters $\omega$ and $v_\text{max}$. We can identify several features. First, when $v_\text{max} = 0$ or when $\omega = 0$ the qubit-loss rate is zero, as expected, since the wall is static in this case. For small values of $v_\text{max}$ the qubit-loss rate is small irrespective of the value of $\omega$. This is the adiabatic regime where the wavefunction of the system closely follows the ground state of the instantaneous Hamiltonian. However, for velocities larger than a critical velocity $v_\text{crit} = |\Delta|$ the qubit-loss rate is large, even for small frequencies $\omega$. This is consistent with the results of Ref. \onlinecite{Karzig2013,Scheurer2013}. In Fig.~\ref{fig:OmegaQubitLoss}(a) we see that the rate of qubit-loss is highest when the wall oscillation frequency $\omega$ is close to the gap energy $E_\text{gap} = \Delta k_F$. This is verified in Fig.~\ref{fig:OmegaQubitLoss}(b), where we plot a cross-section of
Fig.~\ref{fig:OmegaQubitLoss}(a) at a fixed sub-critical value of $v_\text{max}$ for different values of the superconducting gap $\Delta$, and hence different values of the gap $E_\text{gap} = \Delta k_F$. Fig.~\ref{fig:OmegaQubitLoss}(b) also shows that for $\omega \gg E_\text{gap}$, the qubit-loss rate decreases quickly. We find numerically that this drop off is proportional to $1/\omega^4$.
\begin{figure*}[t]
\centering
\includegraphics[width=2\columnwidth]{fig_3.png}
\caption{ (Colour online) (a) Qubit-loss for $v_\text{max} > v_\text{crit}$ (left panel) and $v_\text{max} < v_\text{crit}$ (right panel). The corresponding wall velocity profiles are plotted above. We see that the final qubit loss is larger for two moving walls than for a single moving wall (blue lines vs. red lines) (Plotted for $\Delta = 0.4$). (b) The final qubit-loss at some time $t_\text{fin}$ after the walls have come to rest, plotted as a function of $\tau = 1/\omega$ (for $v_\text{max}=0.1$ and $T=30$). (c) The final qubit-loss in the limit of sudden wall acceleration ($\tau \to 0$). As $T$ gets large we see a sharp distinction emerge between the $v_\text{max}>v_\text{crit}$ and $v_\text{max}<v_\text{crit}$ regimes (here, $v_\text{crit} = |\Delta| = 0.2$). [Other parameters: in all figures, $a=0.5$, $m=0.5$, $L = 200$, $\mu = 1.0$ (in the topological region).]}
\label{fig:P_loss_MBS_transport}
\end{figure*}
\subsection{Qubit-loss in MBS transport}
\label{sect:Adiabatic_Qubit_Loss}

While the frequency $\omega_\text{max}$, at which we have maximum qubit-loss rate, grows with $\Delta$, the actual qubit-loss rate $\langle dP_\text{loss}/dt \rangle_{\text{max}}$ decreases [see insets of Fig.~\ref{fig:OmegaQubitLoss}(b)]. This decrease can be partially put down to the fact that the overall rate of qubit loss depends on the oscillation amplitude. For the choice of parameterisation given in Eq.~\eqref{eq:v_wall_osc} we have \mbox{$x^{(1)}_\text{wall}(t) = x^{(1)}_\text{wall}(0) + v_\text{max}[1 - \cos(\omega t)]/\omega$} and thus for fixed maximum velocity we have a smaller oscillation amplitude at higher frequencies. In similar calculations (not shown) where the wall movement is parameterised as $x(t) = x_0 + x_{\text{max}}\cos( \omega t)$, i.e., with a fixed amplitude $x_\text{max}$, we see the drop-off in qubit-loss rate for $\omega \gg E_\text{gap}$ scale as $1/ \omega^2$.

For fixed frequencies larger than the gap [see e.g., $\omega \approx 0.6$ in Fig.~\ref{fig:OmegaQubitLoss}(b)] we see that the rate of qubit-loss increases as $\Delta$ is increased. This is in contrast to the situation in the low frequency adiabatic regime, where increasing $\Delta$ (hence increasing the gap $E_\text{gap}$) decreases the rate of qubit-loss. Thus while it makes sense to try to maximise the topological gap to counteract low-frequency noise and/or errors associated with deliberate motion of the topological boundary, the situation is more complicated if the range of perturbing frequencies extends above the frequency corresponding to the bulk gap.

\subsubsection{A single moving wall}

The oscillating velocity profile of Eq.~\ref{eq:v_wall_osc} is unsuitable if the goal is to transport a MBS between two different positions on the wire. To model transport, we consider a velocity profile of the form:

\begin{equation}
v_\text{wall}^{(1)}(t) = \begin{cases}
v_\text{max}\frac{1-\cos(\omega t)}{2} & 0 \leq t \leq \frac{\pi}{\omega} \\
v_\text{max} & \frac{\pi}{\omega} \leq t \leq \frac{\pi}{\omega} + T \\
v_\text{max}\frac{1-\cos(\omega t - \omega T)}{2} & \frac{\pi}{\omega} + T \leq t \leq \frac{2\pi}{\omega} + T  \\
0 & \text{otherwise}.
\end{cases}
\label{eq:v_wall_1}
\end{equation}

\noindent This results in an acceleration from zero velocity to a maximum velocity $v_\text{max}$, followed by a period $T$ at constant velocity, and finally a deceleration back to zero velocity [see Fig.~\ref{fig:P_loss_MBS_transport}(a), top panels]. A small frequency $\omega$ corresponds to a slow acceleration of the wall, while a large value corresponds to sudden acceleration.

The qubit-loss due to a single moving wall for MBS transport has been studied in several previous works\cite{Karzig2013,Scheurer2013,Bauer2018}, where it was found that there is a critical velocity $v_\text{crit} = |\Delta|$, below which qubit-loss can be avoided for sufficiently slow acceleration of the wall. Above the critical velocity, qubit-loss will occur even if the acceleration is small \cite{Scheurer2013}. The difference between the $v < v_\text{crit}$ regime and the $v > v_\text{crit}$ regime is revealed by comparing the left and right panels in Fig.~\ref{fig:P_loss_MBS_transport}(a). We see that at some time $t_\text{fin}$ after the wall movement has ended, the final qubit-loss $P_\text{loss}(t_\text{fin})$ is small if $v_\text{max} < v_\text{crit}$, but can be very large if $v_\text{max} > v_\text{crit}$.

We note that in the $v < v_\text{crit}$ regime, the motion is by no means adiabatic (except at very low velocity) and there is considerable qubit loss during the wall's motion in the acceleration phase. However the system returns to the ground state manifold as the wall is slowed down again. This means the wall can be moved far faster than what would be naively considered adiabatic, without permanent qubit loss. This has also been noted in earlier works on this subject\cite{Karzig2013,Scheurer2013} and it is linked to the notion of super-adiabaticity, where the motion can be considered adiabatic in a moving frame  (see e.g Ref. \onlinecite{Berry1987}). We explore this further in Appendices \ref{sect:CriticalVelocityAppendix} and \ref{sect:EffectiveWallMass} where we note that it is possible to think of  the instantaneous energy increase as a kinetic energy of the boundary wall. The final excess energy after the wall has stopped is a small correction to this behaviour, vanishing exponentially with increasing $\Delta$ and $\tau$.

\begin{figure*}[t!]
\includegraphics[width=2.2\columnwidth]{bit_flip_error1.png}

\caption{(Colour online) (a) The density wave packet generated by a \emph{single} moving wall at $x_\text{wall}^{(1)}$ travels at a velocity approximately equal to $v_F$. We can see the wave tunnelling through the non-topological barrier separating the topological phases (barrier height $\mu_\text{barrier} = -2.5$). Here, $v_{\text{max}}=0.3$, and $\omega =3$. (b) The bit-flip error $P_\text{bit}$ increases suddenly as the excitation produced by the movement of one wall hits another moving wall (legend shows which walls are in motion). The time at which the error begins to increase can be estimated as approximately $t \approx |x_\text{wall}^{(i)} - x_\text{wall}^{(j)}| / v_F$ where $|x_\text{wall}^{(i)} - x_\text{wall}^{(j)}|$ is the distance between the two moving walls. [Other parameters for both figures: $m=0.5$, $a=0.5$, $\Delta = 0.4$, $L=200$, and $\mu = 1.0$ (in the topological region).]}
\label{fig:bit_flip_error}
\end{figure*}

To see the dependence of the qubit-loss on the wall acceleration, in Fig.~\ref{fig:P_loss_MBS_transport}(b) we plot the final qubit-loss $P_\text{loss}(t_\text{fin})$ as a function of $\tau = 1/\omega$ in the subcritical $v<v_\text{crit}$ regime. For large $\tau$, corresponding to slow wall acceleration, we see that the qubit-loss follows an exponential decay (in agreement with the results of Ref. \onlinecite{Scheurer2013}). However, the behaviour is different in the region where $\tau \to 0$, corresponding to sudden movement of the wall. In this limit, the qubit-loss reaches its maximum value (for a given $v_\text{max} < v_\text{crit}$). Nevertheless this maximum qubit-loss is usually small and decays with increasing $\Delta$ and we conclude that there is no critical acceleration analogous to the critical velocity in this set-up.

In Fig.~\ref{fig:P_loss_MBS_transport}(c) we plot the qubit-loss as a function of $v_\text{max}$ when $\tau \to 0$ (i.e., in the limit of sudden acceleration). As the time $T$ spent at at the maximum velocity increases we see a sharp distinction emerge between the $v_\text{max} > v_\text{crit}$ and $v_\text{max} < v_\text{crit}$ regimes: for \mbox{$v_\text{max}>v_\text{crit}$} the qubit-loss approaches unity and all theinformation is lost into bulk states, while for $v_\text{max}<v_\text{crit}$ we have $P_\text{loss}(t_\text{fin}) < 1$. This provides further evidence for the interpretation of $v_\text{crit} = |\Delta|$ as a critical velocity.

\subsubsection{Correlated movements and effective wall mass}

We also consider the motion of two boundary walls (the two leftmost walls at $x_\text{wall}^{(1)}$ and $x_\text{wall}^{(2)}$), both by identical velocity profiles $v_\text{wall}^{(1)}(t) = v_\text{wall}^{(2)}(t)$ given by Eq.~\ref{eq:v_wall_1}, so that the two walls are moving in sync and the length of the wire remains constant, see e.g.~Ref.~\onlinecite{Scheurer2013}.

The numerical results shown in Fig.~\ref{fig:P_loss_MBS_transport}(a) show that there is no advantage to coordinated wall movement, compared to a single moving wall. Indeed in the right-panel of Fig.~\ref{fig:P_loss_MBS_transport}(a) we see that for $v_\text{max}<v_\text{crit}$ the qubit-loss is approximately a factor of two higher in this case than for a single moving boundary wall, and that this factor of two persists throughout the movement protocol. In appendix \ref{sect:EffectiveWallMass} we provide a further discussion of the same phenomena where, instead of qubit-loss, we examine the energy above the instantaneous ground state. We find that, up to small exponential corrections due to changes in velocity, the energy increase scales as $\frac{1}{2} M v^2$ where the effective mass scales as  $M \propto p_F^2/E_{\text{gap}}$.

\section{Undetectable qubit errors}
\label{sect:secodaryerrors}

\subsection{Bit-flip error}
\label{sect:BitflipError}
In section \ref{sect:QubitLoss} we saw that the movement of the boundary wall can lead to qubit-loss that can be recovered, to some extent, when $v<v_{\text{crit}}$. This raises the question: can the system return to the qubit space with an error? In this section we will show that bit-flip errors can indeed occur, and we will explore how they are related to excitations produced during the wall movement.

First, we note that, in general, wall movement generates local excitations because of the local nature of the perturbation. These local excitations can then propagate through the wire over time. To investigate this, we consider a single wall (at the position $x_\text{wall}^{(1)}$) oscillating sinusoidally as in Eq.~(\ref{eq:v_wall_osc}) [although similar results can be obtained with the shuttling movement protocol given by Eq.~(\ref{eq:v_wall_1})]. In Fig.~\ref{fig:bit_flip_error}(a) we plot the deviations from the ideal particle density:
\begin{equation}
{\Omega_{j}}(t) = \bra{\psi(t)} c_j^\dagger c_j \ket{\psi(t)} - \bra{\psi_\text{ideal}(t)} c_j^\dagger c_j \ket{\psi_\text{ideal}(t)}, \label{eq::mode}
\end{equation}
as a function of time $t$ and the position $x=ja$ along the wire, due to the motion of the boundary wall. The plot clearly shows a particle density wave that propagates across the wire. The velocity of the propagating wave can be read off from the plot and is found to be approximately equal to the Fermi velocity $v_F$. This value for the velocity is essentially due to the fact that if we consider the system in the moving frame, excitations, made out of quasiparticle and quasiholes with relative momentum $2k_F$, are favoured energetically (see Appendix \ref{sect:CriticalVelocityAppendix} for more details).
\begin{figure}[t]
\centering
\includegraphics[scale=0.2]{qubiterrors.pdf}
\caption{ (Colour online) (a) Schematic showing how excitations originating at the outer walls can dynamically evolve through the system and cause a bit-flip error ( $\ket{\bar{0}} \leftrightarrow \ket{\bar{1}}$ (b) For the anomalous phase rotation the moving boundary wall generates population transfer between ground states $\ket{\psi_{\pm}}$ and excited states. Energy mismatches between states in the bulk can then drive a rotation that either reinforces or opposes the natural rotation due to the ground state splitting. (c) Schematic of how the zero-mode splitting affects ground and bulk-states (see Eq.~\ref{eq:estatenotation} for explanation of the notation).  Deviations from the natural phase rotation (blue) can occur because some excited states (red) have a phase rotation that acts in the opposite direction. The lowest lying pairs of excited states will have a single fermion transferred from a Majorana mode (here the left edge mode) to an excited bulk mode, which means the splitting in these pairs is the same as the splitting between the Majorana modes in the odd fermionic parity sector, which is opposite to the splitting in the even parity sector which contains the qubit states.  Higher energy states (black) can have the same occupation of the Majorana modes as the ground state and then do not contribute to the phase error as they are split in precisely the same way as the ground states.}
\label{fig:qubiterrors}
\end{figure}

We can now understand a mechanism for the occurrence of bit-flip errors. The excitations generated at a moving wall can travel across the wire, and tunnel through non-topological regions in the wire, carrying information between MBS. The resulting interaction between MBS can, in principle, induce bit-flip errors in the topological qubit. This mechanism is illustrated schematically in Fig.~\ref{fig:qubiterrors}(a). It is important to note that, in order for the MBS to interact with the incoming density wave packet, one of the walls on the other side of the system must also be in motion. If this is not the case, the density wave packet will not be able to dissipate at the wall: it will simply be reflected or transmitted without any chance for the excitation to decay back into the degenerate ground state.

This is verified numerically in Fig.~\ref{fig:bit_flip_error}(b), where we show the bit-flip error $P_\text{bit}$ due to the oscillation of boundary walls (the walls that are moving are indicated in curly brackets in the legend). We see that there is no bit-flip error if a single wall is moved and all other walls remain static. However, if two walls are moved, bit-flip errors $P_\text{bit}$ appear abruptly after some delay. The times at which the bit-flip errors begin to appear can be estimated as the time taken for the propagating wave to reach the other moving wall, i.e., as $t \approx |x_\text{wall}^{(i)} - x_\text{wall}^{(j)}| / v_F$ where $|x_\text{wall}^{(i)} - x_\text{wall}^{(j)}|$ is the distance between the two moving walls. This provides strong evidence that it is the stray excitations propagating along the wire that are responsible for the measured bit-flip error.

\subsubsection{Effects of disorder}\label{sect:Disorder}

\begin{figure}[t!]
\centering
	\includegraphics[scale=0.615]{O11DisorderScansText.pdf}
	\caption{ (Colour online) Bit-flip error is suppressed by adding disorder in the middle of the left-hand wire. Here, the disordered region is of length $\sim 40$, and a shorter localisation length $l$ corresponds to increased disorder. We use $v_\text{max}/v_{\text{crit}} = 0.75$, the middle barrier height is $\mu_\text{barrier} = -2.5$, $\sigma = 2$ and the data is averaged over 20 disorder realizations. [Other parameters used for the figure: $m=0.5$, $a=0.5$, $\Delta = 0.4$, $L=200$, and $\mu = 1.0$ (in the topological region).]}
\label{fig::DisorderScan}
\end{figure}

The central result of the previous section is that bit-flip error can occur in a two wire setup if there is a process whereby a quasi-particle is excited in one wire, tunnels through the barrier to the other wire, and then decays back to the ground state manifold. In order to avoid such a process, one straightforward approach would be to increase the barrier between the wires to prevent inter-wire tunneling. However, within the schemes to manipulate quantum information using wire networks, see for example Ref. \onlinecite{Alicea2011}, one often needs to bring neighboring Majorana modes together, a process which would render the barrier more transparent and which would potentially also excite more propagating quasi-particles. In this section we show that another solution to prevent quasi-particle propagation is to introduce some disorder into the wires themselves.

Naively, we might introduce disorder throughout the wire. However there are downsides to doing this. Firstly, in static scenarios, disorder decreases the gap between the ground state and the bulk excitation spectrum, increasing the bound-state decay length \cite{Brouwer2011,Brouwer2011b,DeGottardi2013} and results in a topological space that is less resilient to qubit-loss. Moreover it has been shown \cite{Karzig2013} that moving the confining potential over a disordered region results in a dramatically lower critical velocity, thus severely hampering the rate at which gates can be mechanically performed.

An effective compromise is to deliberately disorder only the central wire regions. This allows for an effective critical velocity of the wire ends that is equal to the $p$-wave order parameter $\Delta$ while also providing a region where bulk excitations are prevented from propagating, reducing the probability that the excitations originating at one wall can tunnel to another wire. This approach still allows for low barrier transparency and so the original schemes\cite{Alicea2011} for braiding and rotating Majorana pairs can be performed as usual.

In Fig.~\ref{fig::DisorderScan} we present the results of our numerical simulations, where disorder has been introduced in the central regions of both wires.  As earlier, we simulate a scenario where there is an oscillation of two walls $x_{\text{wall}}^{(1)}$ and $x_{\text{wall}}^{(4)}$ in different wires. The figure shows the decrease in probability of bit-flip error as we decrease the localization length $l$ in the disordered region. This indicates that as the disorder is increased, the wave associated with excitations accrued at the boundaries cannot propagate through the wire, and hence the junction, to induce a bit-flip error.

\subsection{Phase corrections in a single wire}
\label{sect:phase_error}

In a two wire setup, phase-flip error can occur in precisely the same way as bit-flip error: excitations originating in one wire tunnel into the other wire and relax to the ground state.  However there is another process through which phase error can occur, which importantly does not involve tunneling between wires. This process is shown schematically in Figs. \ref{fig:qubiterrors}(b) and \ref{fig:qubiterrors}(c). The mechanism relies on the fact that splittings between states in the bulk do not necessarily correspond with the splitting that occurs in the ground-state. In systems that experience continual qubit-loss this can lead to a small but systematic phase error being returned to the qubit space.

A necessary feature here is that pairs of bulk excitations that differ in the occupation of the edge modes have slightly different energies. In non-interacting systems this can only happen if there is also some small splitting in the ground state leading to a natural dynamical oscillation between the $\ket{\psi_{\pm}} = \frac{1}{\sqrt{2}} (\ket{\bar{0}}\pm \ket{\bar{1}})$ states. This rate of oscillation depends on the splittings due to the near zero-modes in both wires such that:
\begin{equation}
\label{eq:naturalrotation}
|\braket{\psi_-}{\psi_+(t)}| =  \sin\left(\frac{\delta (t) }{2}\right)
\end{equation}
with $\delta(t) = \int_0^{t} [E_{\bar{1}}(t') - E_{\bar{0}}(t')] dt'$ depends on the difference in energy between the ground states, and hence is related to the decay length of the Majorana edge states.  In Ref. \onlinecite{Scheurer2013} it was noted that because the decay length of the bound states take on a relativistic like correction in moving frames, this rate of rotation within the ground state space can in addition depend on velocity of the system.

The correction to the phase oscillation that we study here  depends on there being a continual qubit-loss/gain channel between the ground state and excited states. If this is the case then energy mismatches between bulk eigenstate pairs will lead to a systematic deviation from this ``natural" Rabi oscillation.  The mechanism is discussed in more detail in Figs. \ref{fig:qubiterrors}(b) and (c).
\begin{figure}[t]
\includegraphics[scale=0.95]{dEdphidt2.pdf}
\caption{
(Colour online) Main figure and upper inset: Qubit-loss induced deviation from the natural phase oscillation tends to act in the opposite direction to the natural oscillation. The red dots indicate $\mu=.03$ and the green $\mu=1.68$.  Lower inset: The deviation $r(t) =\phi(t)-\delta(t)$ (black) and the slopes of the fitted red lines give $\langle \dot{r} (t) \rangle$.  To generate this figure two wires of lengths $45$ and $40$ were used with an essentially infinite barrier between them. The continuum order parameter was set to $\Delta = 0.4$ in the left wire and $\Delta=0.8$ in the right.  The effective electron mass was set to $m=0.5$ and a lattice constant of $a=0.5$ was used.  The velocity of of the left hand boundary of the left wire was moved according to $v(t)=0.1 \sin( 2 t)$}
\label{fig:phaseresults}
\end{figure}

To analyze the deviation from the natural rotation in Eq.~(\ref{eq:naturalrotation}) we first recall that throughout this manuscript we take the view that parts of a state that leave the ground state space are detectable, and therefore we are interested only in the phase rotation within the ground-state manifold.  We therefore need to calculate the conditional probability that the state $\ket{\psi(t)}$ (where $\ket{\psi(0)} = \ket{\psi_+(0)}$) is measured in the instantaneous ground-state $\ket{\psi_\text{phase}}=\ket{\psi_-(t)}$, given that time-evolved state is projected to the ground state manifold.  This probability is given as
\begin{equation}
R(t) =  {\frac{P_{\text{phase}} (t)}{ 1 - P_{\text{loss}}}}= \frac{|\braket{\psi(t)}{\psi_-(t)}|^2}{|\braket{\psi(t)}{\psi_-(t)}|^2+|\braket{\psi(t)}{\psi_+(t)}|^2}.
\end{equation}
From here, we can calculate the phase rotation angle within the ground-state manifold, giving
\begin{equation}
\sin\left(\frac{\phi(t)}{2}\right)=\sqrt{R(t)},
\end{equation}
and then the difference from the natural rotation angle $\delta(t)$ as
\begin{eqnarray}
r(t) &=& \phi(t) - \delta(t)
\end{eqnarray}

In Figure \ref{fig:phaseresults} we plot the behaviour of $dr/dt$ as a function of the chemical potential $\mu$  and the natural phase oscillation due to the small even splitting in both wires. We see that the rate of this phase deviation opposes the mean splitting between the even-odd pairs $\langle \delta (t) \rangle$ that drives the natural phase oscillation.
The mechanism that we describe here relies on there being differences in energies between bulk even-odd eigen-pairs. In a non-interacting system this is necessarily due to a splitting of the edge modes (making them no longer perfect zero modes). This then also implies that there is a splitting between ground states and, as a result, a natural non-topological rotation within the qubit space.  This process can be counteracted by making the wire longer, as this will reduce the overlap between the edge modes.
The situation is different  in interacting systems because in the presence of interaction, the many particle energy spectrum can no longer be described in terms of single particle modes. One thus expects  that there may not be an even-odd degeneracy for bulk states when interactions are strong, even though the ground state degeneracy is robust due to its topological nature. Indeed there is significant evidence that the even-odd symmetry within higher energy eigen-pairs breaks down in regions where bands with different fermion numbers are energetically similar \cite{Gangadharaiah2011,Goldstein2012, McGinely2017,Miao2017,Kells2015a,Kells2015b}.
It may therefore be possible that phase errors similar to the one described here are possible in the presence of non-adiabaticity and interactions, even though the ground state is essentially degenerate.

\section{Concluding remarks}
\label{sect:Conclusions}
In this paper we have investigated possible sources of errors in a toy model of a topological qubit. Our motivation was to understand how error process can arise due to non-adiabatic variation of system parameters. As such, our analysis excludes errors due to interaction with an external environment, and therefore the results only incorporate a subset of possible error processes. Likewise, our analysis does not attempt to incorporate details of specific physical realisations of Majorana based qubits. However, the simplicity of the $p$-wave model should make it relevant to some degree to more realistic device designs (e.g. tetron and hexon proposals \cite{Plugge2017,Karzig2017}) and scalable architectures built from them\cite{Litinski2018}.

As we have stated throughout the paper, we take the viewpoint that the topological qubit consists of two ground states of the Hamiltonian. This is subtly different to the  alternative view where one understands the qubit as the reduced state of the zero-modes obtained by tracing over all excited modes.  Our perspective aligns with the original schemes for 2D topological computers in which measurement of the fusion channels occur as a projections to the many-body ground-states of the system. As we have seen this perspective implies that the system is, at least initially, protected from local errors.

In this context then then our results specifically show how errors can arise in an isolated topological memory, assuming we have a perfect readout protocol. While this approach may not fully reflect the state of current devices, it is what allows us to resolve how errors propagate in time and to see how initial qubit-loss error can eventually lead to more damaging errors. These errors, even with perfect resolution of the fusion channels, cannot be detected without some conventional error correction protocols and the associated computational overhead. For bit-flip error we have shown that this must necessarily involve some tunneling from one wire to another, but for phase error we demonstrated how this could in principle happen via some local process within one wire. For non-interacting models we argue that this results in a correction to qubit rotation due to finite size splitting, in addition to that due to moving reference frames \cite{Scheurer2013}. In follow up work we aim to assess whether this effect can also be triggered by electron-electron interactions \cite{Coopmans2019}.

\vspace{15pt}

\begin{acknowledgments}
The authors would like to thank Luuk Coopmans, Kevin Kavanagh, Niall Moran, Stephen Nulty, Falko Pientka and  Alessandro Romito for useful discussions and comments.  A.C., D.P. and J.K.S. acknowledge financial support from Science Foundation Ireland through Principal Investigator Awards 12/IA/1697 and 16/IA/4524. A.C. was supported through IRC Government of Ireland Postgraduate Scholarship GOIPG/2016/722. S.D. and G.K. acknowledge support from Science Foundation Ireland through Career Development Award 15/CDA/3240.
\end{acknowledgments}

redpajama_set_name: RedPajamaArXiv


I have a slightly bent lower rear trailing arm (Libra/Spider). The two long tubes are bent in the middle - less than 5 degrees. I will take a photo and post later if needed. Can someone tell me what material these are? Can they be straightened? If so, what process should be used - hot/cold etc?
Are they mk1 arms that use the LR ball joints as pivot?
If factory parts they're carbon steel, although what exact grade not sure.
Should be able to do it cold given it's only a small amount.
How did it happen? Given the relatively high strength of that part i'd be concerned what else might be damaged?
I hope this bend didn't happen during your compliance testing!
Thanks guys. They are the later arms with bushes pressed in. Factory parts. They have plates top and bottom and the tubes have bent where the plating stops. I haven't removed it from the car yet but will be conducting a thorough inspection of everything else when I do.
Sanz. HAHA - compliance testing taken a bit too far.
That makes em mk2a or mk3 type.
You could possibly do it DIY with vice/blocks of wood and a big hammer, though perhaps better to find a local engineering firm/garage/repair shop with a hydraulic press that can straighten it with more precise control.
Thanks Sidewinder. I have access to pressing equipment and a jigging table so I will give it a go. I mainly needed some reassurance that we are working with mild steel.
Does anyone have drawings of the Mk 3 trailing arms? Would save me the trouble of removing the other side to take the necessary measurements.


text:
Information about our study programmes
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New fusion gene identified
Researchers at the University of Bergen have discovered a gene variant that increases the risk of chronic pancreatitis
A newly discovered fusion gene increases the risk for chronic pancreatitis. The altered CEL protein accumulates inside the cells (yellow-green color). Cell nuclei are stained blue.
Karianne Fjeld, UiB
By Karianne FjeldPublished: 18.03.2015
Two genes may merge and obtain altered properties. This is nothing new. Such gene fusions are, however, most commonly associated with cancer development. Researchers at KG Jebsen Center for Diabetes Research have now revealed that this type of mutation also may play a role in chronic pancreatitis, ie persistent inflammation of the pancreas.
The results of the Bergen researchers were published this week in Nature Genetics, the world's leading journal for genetic research. Co-authors are international partners from Germany and France.
From diabetes to pancreatitis
The story began with a search for new genes that can cause diabetes. Eight years ago, researcher Karianne Fjeld and professor Stefan Johansson wondered whether a recently discovered diabetes gene could also affect the risk of other pancreatic diseases. After lengthy and comprehensive investigations the hypothesis finally was proved: a variant of the digestive enzyme carboxyl ester lipase (abbreviated CEL) increases the risk of developing chronic pancreatitis at least five times.
The most common cause of this disease is long-term alcohol abuse. Still, doctors cannot find any apparent explanation in about 20 % of the patients. Recent research has suggested that genetic factors are of particular importance in this patient group, an assumption further confirmed by the findings now published in Nature Genetics.
A well-hidden gene variant
What is special about the newly discovered disease variant is how it has arisen. The CEL gene has simply been merged with a neighbouring gene. This results in a chimeric protein where the "head" originates from one gene and the "tail" from another. As a consequence, the CEL enzyme accumulates inside the cells rather than being transported to the intestine.
Stefan Johansson emphasizes that the work has been very challenging.
-Today we use large-scale methods with a high degree of automation to discover new genetic causes of disease. However, these methods fail to identify the fusion gene because of difficulties in distinguishing it from the normal gene, he explains.
Karianne Fjeld adds that the study had to be based on a combination of pioneering work and classical molecular genetic methods conducted in over 2000 patients.
-This, together with necessary cell culture experiments, is the reason why it took this long to make our results ready for publication, Fjeld continues.
Useful genetic diagnostics
The research project was led by professors Anders Molven and Stefan Johansson, affiliated with Departments of Clinical Medicine and Clinical Science at the University of Bergen. The project has been funded mainly by the Bergen Research Foundation and the Kristian Gerhard Jebsen Foundation.
-Detection of genetic risk factors for chronic pancreatitis provides opportunities to improve diagnostics and may lead to new and more targeted treatment, Molven explains.
-Moreover, this knowledge may prevent the patient from being wrongfully suspected of excessive alcohol consumption. Our research is of general interest because we have showed that modern genetic techniques ignore some parts of our genome. Still, we might also there find important keys to disease! Molven says.
Link to the complete article.
Facts about chronic pancreatitis
The pancreas produces enzymes to the alimentary tract as well as hormones that regulate the level of blood glucose.
Chronic pancreatitis is persistent inflammation of the pancreas. The most common symptom is severe upper abdominal pain.
The disease leads to insufficient production of digestive enzymes, which may result in malnutrition, weight loss, fatigue and, eventually, diabetes.
In Norway, at least 10,000 patients suffer from chronic pancreatitis. There is no cure for the disease, but symptoms can be alleviated.
The CEL gene has merged with its neighbour gene. During this process some DNA is lost. The result is a fusion gene, encoding a chimeric protein.
post@med.uib.no+47 55 58 20 86 Universitetet i Bergen
Det medisinske fakultet
Armauer Hansens hus, Haukelandsveien 28 View campus map


Plato (428/427-348/347 BCE) was a Greek philosopher and mathematician of the Classic Age who founded the Academy of Athens. Noted as a student of Socrates, Plato has distinguished himself as one of the founders of Western philosophy by recording the teachings of his master and his own philosophies in 35 dialogues and 13 letters (some are disputed as spurious). However, this collection features only 25 authentic works from the reproduced source.
Benjamin Jowett is credited for translating these works into English.


Increase in the number of orthopedic surgeries is expected to enhance the growth of canes & crutches market from 2018 to 2025.
The North America & Europe canes & crutches market is expected to reach US$ 5,815.1 Mn in 2025 from US$ 2,740.7 Mn in 2017. The North America & Europe canes & crutches market is estimated to grow with a CAGR of 9.9% from 2016-2025. The market is expected to witness growth during the forecast period, owing to increase in the number of orthopedic surgeries.
The rise in the orthopedic surgeries is majorly driven by the surgeries done for the replacements of knee and hip. The surgeries are also been done for the amputations of the limbs due to the damages and injuries caused in the accidents or due to the various diseases. For instance, according to the U.S. Agency for Healthcare Research and Quality, in United States approximately 600,000 knee replacement surgeries are performed per year. The rise in the conditions such as rheumatoid arthritis (RA) and ankylosing spondylitis (AS) and osteoporosis are driving to the number of the surgeries. For instance, according to a report published in 2018 of Healthline Media, rheumatoid arthritis (RA) affects 41 in every 100,000 people per year and near round 1.3 million Americans have RA.
Moreover, the number of surgeries are expected to be rising to the musculoskeletal disorders that are associated with sports, occupational injuries and age-related dysfunction. For instance, according to Arthritis Foundation, in 2017, approximately 54 million adults have been diagnosed with arthritis. In addition, approximately 300,000 babies and children have arthritis or a rheumatic condition. Also the common type of arthritis diagnosed is osteoarthritis, which affects approximately 31 million Americans. Therefore, according to the data and figures, the demand for canes and crutches as an aid for recovery post an orthopedic surgery is anticipated to increase during the forecast period.
The rise in number of orthopedic surgical procedures, would lead to increase in the use of mobility aids such as canes and crutches. Crutches help an individual to move around without putting any weight on your leg or foot, which helps in the process of early recovery post an orthopedic surgical procedure. A cane is available in various forms, such as folding, quad and offset. A quad cane can be preferred for people who need more stability than a standard single-point cane can offer, but who do not need the full support of other mobility devices such as a walker. Canes & crutches helps in gradually increasing the amount of activity one performs around at home post an orthopedic surgery. Hence, the increase in orthopedic surgeries is anticipated to drive the growth of the canes & crutches market during the forecast period.
Some of the prominent players operating in canes & crutches market in North America and Europe are, Carex Health Brands (Compass Health Brands), DRIVE MEDICAL, mikirad, Ottobock, Cardinal Health, Inc., Mobility+Designed, LLC, GF Health Products, Inc., Medline Industries, Inc., BESCO Medical Co., Ltd., and Ossenberg GmbH.


Kwame is a business lawyer and the founder of the American Negotiation Institute. He is passionate about teaching entrepreneurs and business professionals the art of negotiation so they can get better deals and advance their careers. He is regularly invited to give negotiation seminars and consults with individuals and companies to create and implement powerful negotiation strategies. He also hosts a podcast previously called Negotiation for Entrepreneurs, now called Negotiate Anything, where he interviews successful entrepreneurs and shares powerful persuasion techniques.
Excellent podcast. I took notes from start to finish. Thank you.
Holy smokes! Illuminating podcast. Just fantastic tips. Big takeaway for me: how to tactfully say no. As a consultant, a small business owner, an aspiring speaker, and a project manager, being able to say no is a skill and an art. Thank you for the wonderful podcast.
Crystal, you're welcome! It's great to hear that you found value in this conversation with Kwame. You're so right: saying "no" gracefully is no easy task, but it's essential to good leadership. Be sure to check out Kwame's podcast to keep diving deeper into this topic. He's so generous with his expertise, I'm sure you'll find it worth the time!
Excellent ideas in the category of negotiating with this kind of attitude. It really aspires people who know how to handle difficult circumstances. These tips above will be your key to a successful online business.


text:
Q: Longtable and strange behavior after the last footer Here is a compilable .tex file which makes use of the longtable. I understand that longtable is not strictly necessary here, however my real use case contains much more data. This is just a minimal working example I have concocted for the purposes of this question.
\documentclass[a4paper]{article}
\usepackage{multirow}
\usepackage[margin=2cm]{geometry}
\usepackage{longtable}

\begin{document}
  \begin{center}
    \begin{longtable}{|p{2cm}|p{4cm}|p{8cm}|}
      \caption{Relevant past projects} \\
      \hline
      Project Number & Name & Description \\
      \hline
      \endfirsthead
      \multicolumn{3}{c}{\tablename\ \thetable\ -- Continued from previous page} \\
      \endhead
      \multicolumn{3}{r}{Continued on next page} \\
      \endfoot
      \endlastfoot
      112038 & some project name & \multirow{3}{8cm}{Some project description} \\
      \cline{1-2}
      115274 & some other project name & \\
      \cline{1-2}
      202246 & yet another project name & \\
      \hline
      \label{tab:relevant_projects}
    \end{longtable}
  \end{center}
\end{document}

When I compile this using pdflatex, the resulting file shows a table which has vertical lines extending beyond the last footer:

I do not understand why this occurs. Could anyone please help?

redpajama_set_name: RedPajamaStackExchange


I spend a lot of time with couples planning beautiful and meaningful ceremonies followed by perfect receptions, but most of the time I see couples not giving much consideration to the cocktail hour. It's important to plan how to best take care of guests between the ceremony and reception. This time is generally when the wedding party finishes up all those important photos and the vendors put the final touches on the reception room.
The cocktail hour is when guests mingle with old and new friends, eat and drink a little, and basically get organized, locating any table cards before the reception begins. I suggest couples make the most of this little window of time by introducing the unexpected and provide their guests with a fun and interactive experience.
Good upbeat music is definitely a must whether it be through a DJ or your own playlist, but acoustic performers are a fantastic way to add a little flair to your music selections. How fun would dueling piano players be for your guests to get to watch?
Caricature Artists are always a big hit and the sketches make great party favors. Fortune tellers are another fun experience for all.
Strolling Magicians are one of my favorites. They move through the crowd stopping to perform intricate little tricks that will amaze your guests… "wait, how'd you do that?" will be heard frequently.
Living statues are generally more for the artsy crowd, but who doesn't love a human wonder to look at. Another spin on this idea is a living table directing guests to the most delectable items on the buffet or offering up a flute of champagne from a specially designed skirt.
Another very different take on human art would have to be a mime. They may not be as exciting at magicians, but they can be simply mesmerizing for your guests to watch and join in on the acting.
Live dancers and performers… think fire eaters, hula and belly dancers, flamenco dancers, and aerial silk performers.
I recently had the beautiful Janelle Issis, local belly dancer and So You Think You Can Dance star, at one of my events. The guests absolutely loved her!
Slideshows and videos are a way to welcome your guests warmly and give them a little more of your history and insight into how you and your love came to be.
Meet the Wedding Party… a photo display of all the bridesmaids and groomsmen complete with short but fun to read bios. These displays allow your guests to learn more about the special folks who stood beside you during the ceremony as well as provide a way to cut costs by eliminating the need for wedding programs.
Games… who doesn't like a good game to play while killing some time? Consider trivia cards such as "Who Said It" bride and groom cards or Adlibs with advice for the couple. Date night and anniversary bucket list suggestions are always fun for guests to contribute to. And for outdoor weddings, lawn games are perfect entertainment ideas.
Cigar bars… guys (and gals) love watching professional rollers prepare custom smokes. Make sure to designate an outdoor area away from the main event space to not irritate your other guests.
Secondary portrait photographer… photo booths are great for the silly photos, but guests will find it thoughtful of you to offer the services of a pro to snap a nice photo of them all dolled up. We've all had that moment when we wish we had a good photo from attending an event with our significant other. Consider providing some great wingback chairs or furnishings for this setup.
Comedian… whether professional or a close friend who can rock a crowd… everybody loves to laugh!
As you can see, the ideas can be endless. So get creative and add a little fun to your day!


The Liberal Arts Academy is a place for Students, Teachers, Heads of School, and Policy Makers to re-imagine the meaning of the three aims of education – critical thinking, responsible citizenship and well-roundedness.
We invite your to register, take the pre-test, share feedback and think about setting up a Liberal Arts Club in your community to replicate and refine the experiment sketched here.
The Manifesto presents an integrated vision consisting of the Seven Tools of Critical Thinking, the Seven Disciplines of Citizenship, and the Seven Joys of Life.
Critical thinking is all about prioritization. If you can think of more important questions or better answers, please share them.
Our twenty seven matrices identify the most important concepts across the curriculum and the best ways to teach them.


text:
Radiohead lets fans pick price for new album
Posted on September 30, 2007 by jemimus
Sweet fancy Moses this is awesome!* BB reader Daniel says,
Radiohead has just announced the details for their new album, In Rainbows.
They're only selling it through their website (at least for now), and for the digital download version, they're letting listeners pick their own price for the album – it's literally a donation-based product.
Obviously this is sparking confusion among many, but the only help the website provides are the words "It's up to you."
Link, album's out October 10. To recap: the box set (Glorious thick 12″ vinyl! and "enhanced CD") is $80, but the downloads are name-your-own-price. Some readers are reporting that you get the downloads for free anyway if you buy the box set.
No details on the download file format. Does anyone out there know? DRM-free? MP3s? What bitrate, what quality?
I just bought my copy (download, though I'll probably go back and buy the boxed set, too). I got wonky html on the purchase confirmation screen indicating some code glurbles going on at the online store — not sure if my transaction actually took. Perhaps the shop's overloaded right now, announcement just went live.
This is major, and it's such a slap in the record industry's face. An unsigned superband, treating loyal fans and customers like loyal fans and customers instead of thieves — what a revolutionary concept.
In related news, the band is dismissing a hoax website that duped fans this weekend:
The site — http://www.radioheadlp7.com — launched on Friday with a countdown timer due to reach zero on Saturday morning.
It claimed it would be making a big announcement about the band.
Fans speculated the "Creep" hitmakers were planning to reveal details about their next album.
But a spokesperson for the band has called the Web site a "hoax" and "nothing to do with Radiohead."
Link to SF Gate blog post.
Update: More on the band's unusual indie sales approach in these news and blog reports: Green Plastic (fansite online since 1997) Billboard, Idolatr, FQMB.
But Bob Lefsetz, as usual, sums it up best:
It's not like Radiohead's living in a different world. But they're playing by a different rule book. One that says the money flows from the music, that people have to believe in you, that you've got to treat them right.
Shit, you can barely get a ticket to a Radiohead show. The venues aren't big and the demand is incredible. They're doing it all wrong, don't they see??
Well, obviously they don't.
This is big news. This says the major labels are fucked. Untrustworthy with a worthless business model. Radiohead doesn't seem to care if the music is free. Not that they believe it will be. Because believers will give you ALL THEIR MONEY!
This is the industry's worst nightmare. Superstar band, THE superstar band, forging ahead by its own wits. Proving that others can too. And they will.
Disclaimer: I AM THE HUGEST RADIOHEAD FAN ON THE PLANET. (* Thanks Coop)
IT Crowd Season Two – the sexy finale
The season finale of The IT Crowd aired last week — the sex episode, where Jen ends up working as personal assistant to her lecherous boss, leaving the boys to go all Lord of the Flies. This is probably the funniest episode so far — and remarkably restrained for a sex episode. Hard to believe the season's over already — here's hoping for season three!
Eric adds:
I loved The IT Crowd so much, I went searching for other shows with the same actors. So far, both shows I've sampled have been fantastic. They've been mentioned in comments by BB readers, but never in an actual post:
"Garth Marenghi's Darkplace" is a fantastic show featuring both Richard Ayoade (Moss) and Matt Berry (new this season as Douglas Denholm). It is a send up of 80s horror/scifi — spoofing Dr. Who style production on bad Steven King plotlines. A previous BB reader called it "the single best reason to have a multi-region DVD player".
Another show with Berry in it is "The Mighty Boosh", though he's only in four out of fifteen episodes. However, guess who one of the co-stars is: Noel Fielding, IT Crowd's Richmond. His character in Boosh, Vince Noir, is a too-cool punk zoo keeper, and yes it's as funny as it sounds.
Link to Pirate Bay torrent
(Disclosure: I was an unpaid consultant on series one of The IT Crowd, and my fiancee works at Channel Four)
Previews of IT Crowd episode six
IT Crowd, season 2, episode 5: the boob joke episode
IT Crowd Season 2, Episode 4 — and DVD!
IT Crowd Season 2, Episode 3: Great anti-piracy PSA sendup
IT Crowd Season 2, Episode 2 — keyboard-destroying nerd sitcom
The IT Crowd — season two, episode one
New Movie — Inventing Swear Words 3
At long last, I have finished Inventing Swear Words 3! Choose one of the links below to watch the movie—Stage6 is the best quality.
Inventing Swear Words 3 on Myndflame
http://lads.myspace.com/videos/vplayer.swf
I said in my trailer that I would finish it sometime this summer, and since summer officially ends September 23rd, I feel comfortable saying that I've met my goal. If you haven't seen Inventing Swear Words 1, 2 or the trailer for 3 (which doesn't have anything to do with 3), then click on the "Movies" link above and check them out before watching Inventing Swear Words 3.
I am pleased with how this movie turned out. I literally spent every waking moment when I was not at work on this thing. You know you are spending too much time locked up in your apartment when you look in the mirror one day and are startled at how long your beard has grown. For a while there I was marking time by how long my fingernails had grown. I'm pleased with this movie, but I am also very glad to be joining the real world again and attaining some semblance of normalcy.
I have to give major thanks to Nathan Allen Pinard, who is a true hero of this project. I asked him to complete the sound track in four days, and he did it—and it turned out perfect! He really came through, which is why I was able to release this movie today. So stop on over at Nathan's site and thank him for working on Inventing Swear Words 3.
I have a brand new website! Scott Repka contacted me a few weeks ago and offered to redesign my website, and I must say, it is very handsome–much better than my old Homestead one. The "Writings" section will be updated here in a few days, but in the meantime, check out the new "Movies" page, and the adjacent "Characters" page, where you can find out more about the characters from my videos.
I have updated my store with lots of cool new items! Craig Lynn offered to design some images for me, and with these I was able to flesh the store out with new shirts for men, women and children, including black and dark colored shirts, as well as other odds and ends like mugs, steins, mouse pads, pillows, aprons, magnets, posters, coasters and more. So check out the new store, and see if anything catches your eye!
Well, with that, I think I am going to take a long overdue break. Maybe I'll go hiking this weekend. Or maybe I'll just sleep. I have a few days to decide.


text:
Danielle Trussart (born December 3, 1948) is a visual artist and writer living in Quebec, Canada.

She was born in Montreal, Quebec. Trussart received her teaching certificate from the École normale Jacques-Cartier and went on to study Quebec studies, adult education and special education at the Université de Montréal and the Université du Québec à Montréal. She co-founded an alternative school at Saint-Jérôme and taught at an alternative school in Sainte-Thérèse. She also took workshops in visual arts. Since 1993, she has lived at Baie-Saint-Paul where she operated an inn.

Trussart established a small publishing house to distribute her own illustrations of Quebec folk songs. She exhibits her art in Baie-Saint-Paul and Sainte-Thérèse. She was co-author of a collection of books for children. Trussart has contributed to the literary journals Arcade, Brèves littéraires and L'embarcadère. Her 2008 novel Le train pour Samarcande received the Prix Robert-Cliche.

She received honourable mention in 2005 for a  and was awarded that prize in 2007. In 2006, Trussart was a finalist in the literary competition sponsored by Radio-Canada.

References

1948 births
Living people
Artists from Montreal
Canadian women painters
Canadian novelists in French
Canadian women novelists
Canadian children's writers in French
Université de Montréal alumni
Université du Québec à Montréal alumni
Writers from Montreal
21st-century Canadian painters
21st-century Canadian novelists
21st-century Canadian women artists
21st-century Canadian women writers
Canadian women children's writers

redpajama_set_name: RedPajamaWikipedia


Google is not known to spill the beans on how some businesses highly rank than the others in search engine results. However, paying close attention to what your visitors want from you and keeping track on Google Ranking Algorithm is all you need to do. The first step towards SEO can be scary, but if you start implementing the small changes to your SEO strategy, you will gradually lead towards success. In case you need any help, go for the best SEO services in Delhi.
Now, read on to discover the Google Ranking Factors 2018 which will definitely improve your site's ranking.
Content is one of the most important tools for an enhanced SEO ranking, but in recent years we have seen a vast shift from quality content to keyword focused content. That is the reason why people are not getting the desired results. Repetitive content looks dull and copied content will let you penalized. So, writing high-quality, well-written, well-researched content is the modern approach for SEO.
When SEO teams forget to give page titles that can take a toll on your rankings, posing a negative picture of your website. And the pages with substandard content with long-tail keywords are ranked quite well, because they have titles to their pages. Ring a bell?
With the advent of Pigeon, site owners have learnt to focus on local searches. With over 80% of local searches, immediate purchase decision has been enhanced on a vast scale.
If you think that the designs and outlook of your website are not that important, then you are getting it all wrong. Get your design and development team involved with search optimization. Your webpage must be responsive and built with UI/UX to keep the things organized.
For those who have not done this yet, it's time to educate yourself about the importance of backlinks. The link profile cleanup is the building of your quality backlinks which results in the stronger network of knowledge.
We can't deny the fact that each social channel has its own filter algorithm which lifts great content on the top. So sharing different channels of social media can be beneficial for your content and thus, your website. And if the content is getting clicks, views, and shares, then there is a circle influence happening for sure.
If you have the thin content on your webpage, then start rewriting it or remove it. Provide the well-informatory and unique content to your regular customer and learn the complete guide to double your search traffic via impeccable SEO tips.
In a complicated and competitive field, you need to have a good hold on a variety of detailed subjects. And with these pointers, you are going to rank well in 2018 for sure. Google makes a steady push to rich content, quality links, and a good mobile experience, so you must utilize it. Also, Google's Pigeon Update makes a great impact on local search. If you are still confused with the things, then hire the Best SEO Services in Delhi.


us can Live Without Fear.
13 And who will harm you if you are deeply committed to what is good?
I do not know any Christian who goes around in fear. In the time of this text and several places of our world today some will gladly kill you. In those circumstances these Christian possess an inspiring testimony.
I believe the Christian Pastor who was held for 1,000 days simple because he converted to Christianity and would not recant will be brought over hear to speak. I will try to hear him. It would seem he really has a testimony all of us would be blessed in hearing. He is an example of contentment in Christ. He certainly focused on his blessings in Christ.
15 but honor the Messiah as Lord in your hearts. Always be ready to give a defense to anyone who asks you for a reason for the hope that is in you.
16 However, do this with gentleness and respect, keeping your conscience clear, so that when you are accused, those who denounce your Christian life will be put to shame.
Recently we had a speaker who made a point related to sharing about Christ by showing pictures of family members. He ask how many had taken a course in sharing pictures of family members. No one raised their hand and he made the point sharing pictures comes naturally. Because we love our children, grandchildren.and other family members we share about them naturally. He made the point that we need to be ready to share about Jesus because we love Him and are proud of what He has done for us. The text tells us to do this as we live for Christ and share a good example. We do not want to be accused of not practicing what we preach. We want to walk the walk and talk the talk. We certainly have a reason to share.
18 For Christ also suffered for sins once for all, the righteous for the unrighteous, that He might bring you to God, after being put to death in the fleshly realm but made alive in the spiritual realm.
to the spirits in prison. There ar several suggested interpretations of that in the teachers quarterly You need to ask your pastor to share his interpretation of that for you.
20 who in the past were disobedient, when God patiently waited in the days of Noah while an ark was being prepared. In it a few—that is, eight people—were saved through water.
21 Baptism, which corresponds to this, now saves you (not the removal of the filth of the flesh, but the pledge of a good conscience toward God) through the resurrection of Jesus Christ.
22 Now that He has gone into heaven, He is at God's right hand with angels, authorities, and powers subject to Him.
Notice this does not say, "saved by water but through the water." Baptism does not save anyone. It is an act of obedience by people who know they are already saved through their commitment to Christ. Now it does say being baptized does save related to a good conscience toward God. As a Christian you cannot refuse to be baptized and possess a clear conscience before God. He commanded us to be baptized. Verse 22 gives the picture of Christ in heaven with all of the powers of heaven and earth subject to Him. What a sight for us to behold in person someday as we will be Living Without Fear. Amen? Amen!


text:
<?xml version="1.0" encoding="UTF-8"?>

<blueprint xmlns="http://www.osgi.org/xmlns/blueprint/v1.0.0"
	xmlns:xsi="http://www.w3.org/2001/XMLSchema-instance"
	xsi:schemaLocation="
		http://www.osgi.org/xmlns/blueprint/v1.0.0 http://www.osgi.org/xmlns/blueprint/v1.0.0/blueprint.xsd">

	<description>Importer configuration</description>

	<reference id="simple" interface="java.lang.Cloneable" />

	<bean id="listener" class="org.springframework.osgi.blueprint.ImporterListener" />

	<reference id="options" interface="java.io.Serializable"
		availability="optional" component-name="foo" filter="(name=foo)">
		<reference-listener bind-method="bind" unbind-method="unbind" ref="listener" />
	</reference>

	<reference id="multipleInterfaces" interface="java.lang.Cloneable"/>

	<reference id="multipleListeners" interface="java.lang.Cloneable">
		<reference-listener bind-method="bindM" unbind-method="unbindM" ref="listener" />

		<reference-listener bind-method="up" unbind-method="down">
			<bean class="org.springframework.osgi.blueprint.ImporterListener" />
		</reference-listener>
		<reference-listener bind-method="refBind" unbind-method="refUnbind">
			<ref component-id="listener" />
		</reference-listener>
	</reference>

	<reference id="timeout" interface="java.lang.Cloneable"
		timeout="1234" />

    <!-- promoted beans should be hidden to the Blueprint API -->
    <!--  the nested property should be reflected as a nested component rather then a reference to a top level bean -->
    <bean id="nestedReference" class="org.springframework.osgi.blueprint.TestComponent" init-method="init">
       <property name="propA">
           <reference interface="java.io.Serializable" timeout="1000"/>
       </property>
    </bean>

     <bean id="nestedCollectionReference" class="org.springframework.osgi.blueprint.TestComponent" init-method="init">
       <property name="propA">
           <reference-list interface="java.io.Serializable" member-type="service-reference"/>
       </property>
    </bean>

</blueprint>

redpajama_set_name: RedPajamaGithub